---
abstract: 'Mass accretion onto (proto-)stars at high accretion rates $\dot{M}_\ast > 10^{-4}~M_{\odot}~{\rm yr}^{-1}$ is expected in massive star formation. We study the evolution of massive protostars at such high rates by numerically solving the stellar structure equations. In this paper we examine the evolution via disk accretion. We consider a limiting case of “cold” disk accretion, whereby most of the stellar photosphere can radiate freely with negligible backwarming from the accretion flow, and the accreting material settles onto the star with the same specific entropy as the photosphere. We compare our results to the calculated evolution via spherically symmetric accretion, the opposite limit, whereby the material accreting onto the star contains the entropy produced in the accretion shock front. We examine how different accretion geometries affect the evolution of massive protostars. For cold disk accretion at $10^{-3}~M_{\odot}~{\rm yr}^{-1}$ the radius of a protostar is initially small, $R_\ast \simeq$ a few $R_\odot$. After several solar masses have accreted, the protostar begins to bloat up and for $M_\ast \simeq 10~M_\odot$ the stellar radius attains its maximum of $30 - 400~R_\odot$. The large radius $\sim$$100~R_\odot$ is also a feature of spherically symmetric accretion at the same accreted mass and accretion rate. Hence, expansion to a large radius is a robust feature of accreting massive protostars. At later times the protostar eventually begins to contract and reaches the Zero-Age Main-Sequence (ZAMS) for $M_\ast \simeq 30~M_\odot$, independent of the accretion geometry. For accretion rates exceeding several $10^{-3}~M_{\odot}~{\rm yr}^{-1}$ the protostar never contracts to the ZAMS. The very large radius of several $100{\rm s}~R_\odot$ results in a low effective temperature and low UV luminosity of the protostar. Such bloated protostars could well explain the existence of bright high-mass protostellar objects, which lack detectable H II regions.'
author:
- 'Takashi Hosokawa, Harold W. Yorke, Kazuyuki Omukai'
bibliography:
- 'refs.bib'
title: Evolution of Massive Protostars via Disk Accretion
---

Introduction {#sec:intro}
============

Recent studies have revealed that the formation process of massive $(> 8~M_\odot)$ stars differ in many respects from that of low-mass $(\sim 1~M_\odot)$ stars (e.g., Zinnecker & Yorke 2007). Although signatures of mass accretion are widely observed toward forming massive stars, the estimated accretion rates usually exceed $10^{-4}~M_{\odot}~{\rm yr}^{-1}$, which are much higher than the typical value in low-mass star formation, $$\dot{M}_\ast \sim \frac{c_s^3}{G} \simeq
5 \times 10^{-6} \left( \frac{T}{10~{\rm K}} \right)~
M_\odot~{\rm yr}^{-1},
\label{eq:lmass_acc}$$ where $c_s$ and $T$ is the sound speed and temperature in natal molecular cloud cores, and $G$ is the gravity constant. In the past it has been argued that such high accretion rates are required for accretion flow to overcome the strong radiation pressure from forming massive stars (e.g., Larson & Starrfield 1971; Wolfire & Cassinelli 1987). However, these results were based on the assumption of spherically symmetric infall. Nevertheless, there are other good reasons to expect high accretion rates during the formation of massive stars: Massive stars have short Kelvin-Helmholz time scales, once formed they consume the available nuclear fuel quickly, and they will lose a significant part of their mass through strong stellar winds. Thus, massive stars evolve quickly, even while accreting. We can expect the time spent in the main accretion phase to be significantly less than the main sequence lifetime, presumably of the order of a few dynamical times of the star-forming molecular core. For a $30~M_\odot$ star this provides a lower limit to the average accretion rate $\simeq 10^{-4}~M_{\odot}~{\rm yr}^{-1}$. Accretion rates may vary strongly, however. Thus, phases of even higher accretion rates are likely.

The high accretion rates suggest that the nature of massive star formation differs from that of low-mass star formation. So far, various formation scenarios, such as monolithic collapse of massive dense cores (e.g., Yorke & Sonnhalter 2002; McKee & Tan 2002, 2003; Krumholz et al. 2007, 2009), and the competitive accretion with global infall of the cluster-forming clumps (e.g., Bonnell et al. 1998; Bonnell, Vine & Bate 2004; Wang et al. 2010), have been proposed. The proposed formation scenarios are being assessed with high-resolution observations of the massive cores and clumps (e.g., Motte et al. 2007; Marseille et al. 2008; Zhang et al. 2009; Bentemps et al. 2010).

The evolution of massive protostars at such high rates is a critical feature of massive star formation which determines the effect these stars have on their environment (e.g., Zinnecker & Yorke 2007). In our previous work (Hosokawa & Omukai 2008; 2009, hereafter Paper I), we examined the evolution by numerically solving the interior structure of a protostar with a dusty accretion envelope under the assumption of spherical symmetry. Our calculations show that accreting massive protostars have certain characteristic features. At $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$, for example, the protostellar radius becomes very large, exceeding $100~R_\odot$ at maximum. The evolution before the arrival to the zero-age main sequence (ZAMS) lasts until $M_\ast \simeq 30~M_\odot$. At even higher accretion rates $\dot{M}_\ast > 3 \times 10^{-3}~M_{\odot}~{\rm yr}^{-1}$, the protostar very abruptly inflates and overtakes material in the inner part the accreting envelope, thus invalidating the assumption of steady mass accretion before reaching the ZAMS.

The very large stellar radius leads to a low effective temperature of the protostar, which in turn explains some observational properties of massive protostars in Orion KL nebula (Morino et al. 1998; Furuya & Shinnaga 2009).

Observations suggest that mass accretion onto massive stars is not spherically symmetric, but rather proceeds through massive circumstellar disks (e.g., Cesaroni et al. 2007). Signatures of rotating infall are widely found toward forming massive stars, sometimes associated with massive outflows along the rotation axis (e.g., Patel et al. 2005; Beltrán et al. 2006a). Recent numerical simulations also suggest that the massive disk is a natural outcome of collapse of a massive dense core (Yorke & Sonnhalter 2002; Krumholz et al. 2007, 2009). Protostellar evolution via disk accretion has been studied for lower-mass protostars with low accretion rates $\dot{M}_\ast \leq 10^{-4}~M_{\odot}~{\rm yr}^{-1}$ (e.g., Palla & Stahler 1992; Beech & Mitalas 1994; Hartman et al. 1997). These authors considered the limiting case of “cold” disk accretion, whereby most of the stellar surface is able to radiate into free space and the accreting material brings only a small amount of entropy into the star. They showed that, with the low accretion rates, disk accretion slightly reduces the stellar radius compared to the spherically symmetric cases.

Maeder and coworkers studied the evolution of accreting massive protostars in the cold disk limit with mass accretion rates increasing with the stellar mass up to $10^{-4}~M_\odot~{\rm yr}^{-1}$ (e.g., Norberg & Maeder 2000; Behrend & Maeder 2001). Recently, Yorke & Bodenheimer (2008, hereafter YB08) calculated the evolution in the same limit with much higher accretion rates $10^{-3}$ and $10^{-2}~M_\odot~{\rm yr}^{-1}$. Their calculated evolution differs from the spherical accretion case in an early phase of $M_\ast \lesssim 8~M_\odot$. The stellar radius is several 10s$~R_\odot$ with spherical accretion, whereas it is a few $R_\odot$ with disk accretion. However, YB08 find that the stellar radius rapidly increases soon afterwards and exceeds $100~R_\odot$ at $M_\ast \simeq 10~M_\odot$. The subsequent evolution at $M_\ast \gtrsim 10~R_\odot$ is quite similar for both spherical accretion and disk accretion.

In this paper, we examine how the different accretion geometries affect the evolution of massive protostars at high accretion rates. We explain why the two extreme cases lead to the same characteristic features of massive protostars, such as the large radius, in spite of the different evolution in the early phases. To this end, we calculate the protostellar evolution in the cold disk accretion limit with the numerical code used in Paper I. This allows us to extract how the protostellar evolution depends on the different accretion geometry independent of the effects of different stellar evolution codes. For completeness, we also compare the calculated evolution with previous results by YB08.

Finally, we stress that this study is very relevant to star formation in the early universe, where high accretion rates are also expected. Protostellar evolution with high accretion rates has been studied with zero or very low metallicities under the assumption of spherically symmetric accretion (e.g., Stahler, Palla & Salpeter 1986; Omukai & Palla 2001, 2003; Hosokawa & Omukai 2009b). Recent numerical simulations show that circumstellar accretion disks are also expected during star formation in the early universe (Yoshida, Omukai & Hernquist 2008; Stacy, Grief & Bromm 2010). Tan & McKee (2004) examined the evolution of primordial protostars via disk accretion using simple analytic models. Here, we calculate the detailed evolution of a primordial protostar in the cold disk accretion limit.

The organization of this paper is as follows. The numerical method and the cases considered are briefly described in Section \[sec:num\]. In Section \[sec:result\], we focus on the protostellar evolution at the accretion rate $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$, which allows a direct comparison to the results of YB08. First, we briefly review the evolution via spherical accretion studied in Paper I (Section \[ssec:sp\_acc\]), and then consider the evolution via cold disk accretion (Section \[ssec:d\_acc\]). Evolution of a primordial protostar is investigated in Section \[ssec:metal\] and subsequently contrasted to the present-day cases. Variation of the protostellar evolution with different accretion rates is studied in Section \[sec:mdot\_dep\]. Finally, Section \[sec:sum\] is devoted to our summary and conclusions.

Numerical Modeling {#sec:num}
==================

Modeling Mass Accretion via Disks {#ssec:coldisk}
---------------------------------

We examine protostellar evolution by numerically solving the stellar structure equations. Case (a) in Figure \[fig:prost\_schem\_spph\] presents the schematic picture of the spherical accretion studied in Paper I, where we assumed spherical symmetry for an accretion envelope as well as the protostar. The numerical method we adopted is summarized as follows (e.g., Stahler, Shu & Taam 1980; also see Appendix A of Paper I). For a protostar, we solve the four stellar structure equations taking into account mass accretion. Free-fall flow is assumed for the optically thin part of the accretion envelope. If the accretion flow becomes opaque to the stellar radiation before hitting the stellar surface, we solve for the structure of this optically thick part of the flow together with the stellar structure equations of the protostar and the jump conditions at the accretion shock front. The accretion shock front is the outer boundary of the modeled protostar (shock boundary).

For the case of mass accretion via a circumstellar disk we consider the limiting case whereby the disk-star connecting layer is geometrically thin and most of the stellar surface is unlinked to the accretion flow. Figure \[fig:prost\_schem\_spph\] depicts this situation. In this case, the usual photospheric outer boundary condition can be applied for accreting protostars (e.g., Palla & Stahler 1992), $$\label{eq:psb_p}
P_{\rm sf} = \frac23 \frac{1}{\kappa_{\rm sf}} \frac{G M_\ast}{R_\ast^2} ,$$ $$\label{eq:psb_l}
L_\ast = 4 \pi R_\ast^2 \sigma T_{\rm sf}^4 ,$$ where the suffix “sf” indicates the values at the stellar surface, and $\sigma$ is Stefan-Boltzman constant. In this limiting case of disk accretion, accreting materials add to the star with the smallest amount of entropy, which is the value in the stellar atmosphere unattached to the accretion flow. Hence, the treatment with equations (\[eq:psb\_p\]) and (\[eq:psb\_l\]) supposes the limit of “cold” disk accretion. Note that this cold disk accretion is just a limiting case. Gas accreting onto the star through the disk is likely to have somewhat higher entropy especially at high accretion rates (Hartmann et al. 1997). The spherical accretion is the opposite limit where accreting materials carry the highest amount entropy into the star. Thus, we consider two extreme limiting cases with the spherical accretion and cold disk accretion. In order to solve the protostellar structure with cold disk accretion, we modified the numerical code used in Paper I to deal with the photospheric boundary condition. We do not solve the detailed structure of the flow connecting the star and disk.

Different geometries of the accretion flow will lead to different structures of the evolving protostar. For example, the average entropy in the stellar interior reflects the history of entropy brought into the star with accreting material, which in turn depend on the accretion geometry. For spherical accretion at high accretion rates the accretion shock front is embedded inside the stellar photosphere and most of the high entropy created at the accretion shock front is carried to the stellar surface. This entropy is efficiently taken into the stellar interior with high accretion rates (Paper I). As a result the protostar has a higher average entropy (compared to a non-accreting protostar), which leads to a very large radius – exceeding $100~R_\odot$ at maximum. With disk accretion, however, entropy is mainly generated within the disk by viscous dissipation. Before the accreted material reaches the stellar surface, a large fraction of the generated entropy will be transported away by radiation. As a result, entropy brought into the star with the accreting material is significantly lower than in the spherical accretion case. The average entropy within the star $s$ is related to the stellar radius as $$R_{\ast} \propto M_{\ast}^{-1/3}{\rm exp}[const. \times s].
\label{eq:r_entropy}$$

This relation is derived by substituting the typical gas density and pressure within a star of mass $M_{\ast}$ and radius $R_{\ast}$ (e.g., Cox & Giuli 1968); $$\rho \sim \frac{M_{\ast}}{R_{\ast}^3},
\qquad P \sim G \frac{M_{\ast}^2}{R_{\ast}^4},
\label{eq:typ_rhop}$$ to the definition of specific entropy of ideal monotonic gas, $$s = \frac{3 \cal{R}}{2 \mu} \ln \left( \frac{P}{\rho^{5/3}} \right) + const.,
\label{eq:s_gene}$$ where ${\cal R}$ is the gas constant and $\mu$ is the mean molecular weight. Equation (\[eq:r\_entropy\]) demonstrates that, for the same stellar mass, the stellar radius is larger with the higher average entropy in the stellar interior. Thus, we can naively expect that the stellar radius is reduced with disk accretion. Contrary to this expectation, however, calculations by YB08, adopting the cold disk accretion, show that the radius of a massive protostar exceeds $100~R_\odot$ at maximum as with the spherical accretion. The goal of this paper is to explain why the outcomes are so similar among the extreme cases of the spherical accretion and cold disk accretion.

\[tb:md\]

Table 1. Input Parameters of the cases considered\

  Case                $\dot{M}_\ast~(M_{\odot}/{\rm yr})^a$   geometry    $Z^c$   $M_{\ast,0}~(M_{\odot})^d$   $R_{\ast,0}~(R_{\odot})^e$             reference$^f$
  ------------------ --------------------------------------- ----------- ------- ---------------------------- ---------------------------- ------------------------------------ --
  MD4x3-SDm0.5$^g$             $4 \times 10^{-3}$             S $\to$ D   0.02            0.3 (0.5)                   32.7 (36.8)               Section \[sec:mdot\_dep\]
  MD4x3-S                      $4 \times 10^{-3}$                 S       0.02               0.3                          32.7              Section \[sec:mdot\_dep\], Paper I
  MD3-D                             $10^{-3}$                     D       0.02               0.1                          3.7                    Section \[ssec:d\_acc\]
  MD3-D-b0.1                        $10^{-3}$                     D       0.02               0.1                          3.5                     Section \[sssec:imod\]
  MD3-D-cv                          $10^{-3}$                     D       0.02               1.3                          6.2                     Section \[sssec:imod\]
  MD3-S                             $10^{-3}$                     S       0.02               0.05                         15.5              Section \[ssec:sp\_acc\], Paper I
  MD3-S-z0                          $10^{-3}$                     S        0.0               0.05                         13.0               Section \[ssec:metal\], Paper I
  MD3-SDm1                          $10^{-3}$                 S $\to$ D   0.02            0.05 (1.0)                  15.5 (24.4)                 Section \[sssec:imod\]
  MD3-SDm0.1                        $10^{-3}$                 S $\to$ D   0.02            0.05 (0.1)                  15.5 (14.1)                 Section \[sssec:imod\]
  MD3-SDm0.1-z0                     $10^{-3}$                 S $\to$ D    0.0            0.05 (0.1)                  13.0 (14.1)                 Section \[ssec:metal\]
  MD4-S                             $10^{-4}$                     S       0.02               0.03                         8.8               Section \[sec:mdot\_dep\], Paper I
  MD4-SDm0.1                        $10^{-4}$                 S $\to$ D   0.02            0.03 (0.1)                   8.8 (5.1)                Section \[sec:mdot\_dep\]
  MD4-D-cv                          $10^{-4}$                     D       0.02               1.3                          6.2                     Appendix \[ap:cp\_ps\]
  MD5-D-cv                          $10^{-5}$                     D       0.02               1.0                          4.3                     Appendix \[ap:cp\_ps\]
  MD5-S-cv                          $10^{-5}$                     S       0.02               1.0                          4.2                Appendix \[ap:cp\_ps\], Paper I

$a$ : mass accretion rate, $b$ : geometry of the accretion flow (D: disk accretion, S: spherical accretion), $c$ : metallicity, $d$ : mass of initial core model, $e$ : radius of initial core model, $f$ : subsections where numerical results of each case are presented. $g$ : the suffix SDm$X$ means the geometry is switched from spherical accretion to disk accretion at $M_\ast = X~M_\odot$. For these cases, stellar mass and radius at the switching point are listed in the brackets in the columns of $M_{\ast,0}$ and $R_{\ast,0}$.

Cases considered
----------------

Table 1 summarizes the cases considered in this study and their input parameters. For simplicity the protostellar evolution is calculated with a constant given accretion rate for each case. The adopted accretion rates range from $10^{-5}~M_\odot~{\rm yr}^{-1}$ up to $4 \times 10^{-3}~M_\odot~{\rm yr}^{-1}$. Evolution for the accretion rate $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$ is studied in detail. In addition to evolution with cold disk accretion we present several cases with spherical accretion for comparison. Evolution via disk accretion at the rates $\dot{M}_\ast = 10^{-5}~M_{\odot}~{\rm yr}^{-1}$ and $10^{-4}~M_{\odot}~{\rm yr}^{-1}$ was also studied by Palla & Stahler (1992). We consider protostellar evolution with these low rates to compare our results with theirs (see Appendix \[ap:cp\_ps\]).

The initial model in each case is constructed following Stahler, Shu & Taam (1980) or Palla & Stahler (1991) with the adopted accretion rate and boundary conditions (also see Appendix A.2 and B.2 in Paper I). The initial stellar mass $M_{\ast,0}$ is taken as an arbitrary small value. The initial entropy profile in the stellar interior is assumed as a function of the mass coordinate $M$, $$s(M) = s_{c,0}
+ \beta \frac{k_{\rm B}}{m_{\rm H}} \frac{M}{M_{\ast,0}} ,
\label{eq:s0}$$ where $s_{c,0}$ is specific entropy at the stellar center, $k_{\rm B}$ is Boltzmann constant, $m_{\rm H}$ is atomic mass unit, and $\beta~(> 0)$ is a free parameter. We adopt $\beta = 1$ as a fiducial value. Unlike the cases of spherical accretion, however, we will see that the protostellar evolution with the photospheric boundary changes with different initial models even at the same accretion rate (see Section \[sssec:imod\] below). We show this by presenting the evolution with different initial models with $\beta = 0.1$ (shallower entropy profile, case MD3-D-b0.1), and $\beta = 0$ (homogeneous entropy profile, cases with the suffix “cv”).

The geometry of the accretion flow will vary as a function of the stellar mass and radius. Initially, the collapse of a gravitationally unstable molecular core is mostly spherically symmetric. A hydrostatic object is formed when the central regions of the molecular core become optically thick. A circumstellar disk is later formed as material with increasingly higher angular momentum falls toward the newly formed protostar. For these cases we start the protostellar evolution calculation assuming spherical accretion and later switch to cold disk accretion (cases with the suffix “SD”). We also present the evolution of primordial protostars via disk accretion (case MD3-SDm0.1-z0).

Evolution of Massive Protostars with $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$ {#sec:result}
=====================================================================================

Spherically Symmetric Accretion {#ssec:sp_acc}
-------------------------------

Here, we briefly review the evolution with spherically symmetric accretion studied in Paper I. The upper panel of Figure \[fig:str\_log\_1em3b1\_sh\] shows the evolution of the stellar radius and interior structure at the accretion rate $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$ (case MD3-S). We define the following four evolutionary phases from the behavior of the stellar radius: (I) gradual expansion ($M_\ast \lesssim 6~M_\odot$), (II) swelling ($6~M_\odot \lesssim M_\ast \lesssim 10~M_\odot$), (III) contraction ($10~M_\odot \lesssim M_\ast \lesssim 30~M_\odot$), (IV) gradual expansion ($M_\ast \gtrsim 30~M_\odot$). A key quantity to understand the variety of the evolution is the ratio between the accretion timescale, $$t_{\rm acc} \equiv \frac{M_{\ast}}{\dot{M}_\ast} ,$$ and the Kelvin-Helmholtz (KH) timescale, $$\label{eq:tkh}
t_{\rm KH} \equiv \frac{G M_{\ast}^2}{R_{\ast} L_{\ast}} .$$ The former is the evolutionary timescale, and the latter is the timescale over which a star loses energy by radiation. The lower panel of Figure \[fig:str\_log\_1em3b1\_sh\] displays the evolution of these timescales. We see that $t_{\rm KH}$ significantly decreases during phase (II). As a result, the balance of these timescales changes from $t_{\rm acc} \ll t_{\rm KH}$ in phase (I) to $t_{\rm acc} > t_{\rm KH}$ in phase (III) and (IV). The decrease of $t_{\rm KH}$ is caused by a rapid increase of the stellar luminosity $L_\ast$, which in turn is a result of the decrease in opacity. In most of the stellar interior the opacity’s dependence on density and temperature is approximated by Kramers’ law $\kappa \propto \rho T^{-3.5}$. Thus, as the stellar mass increases, the temperature in the interior rises and the opacity decreases.

Figure \[fig:slpf\_1em3\_sh\] shows snapshots of radial profiles of entropy and luminosity in the early phases (I) and (II). At the assumed high accretion rate the entropy is initially efficiently brought into the stellar interior with minimal radiative loss because of the high opacity during phase (I). The instantaneous entropy profile simply traces the post-shock values from earlier times (adiabatic accretion). The average entropy within the star increases with accreted mass, which according to equation (\[eq:r\_entropy\]) means that the stellar radius should also grow. This is indeed the case in phases (I) and (II). As the average density decreases and the temperature increases, the opacity decreases; radiative heat transport becomes more efficient with increasing stellar mass.

For $M_\ast \gtrsim 6~M_\odot$ (phase II) radiative heat transport is efficient enough to modify the entropy distribution within the star. The deep interior (where $\partial L/ \partial M > 0$) loses entropy, whereas the outer surface regions (where $\partial L/ \partial M < 0$) gain a significant amount of entropy. This gain in entropy results in the “bloating up” of the star up to $\gtrsim100~R_\odot$ at maximum. Figure \[fig:slpf\_1em3\_sh\] shows that the boundary between the heat-losing interior and heat-gaining outer layer, namely where $\partial L/\partial M = 0$, moves toward the stellar surface with increasing stellar mass. Stahler, Palla & Salpeter (1986) called this characteristic behavior of luminosity profiles a “luminosity wave”. The stellar surface luminosity $L_\ast$ rapidly increases when the luminosity wave approaches the stellar surface. After the luminosity wave passes through the surface, the star can efficiently lose energy by radiation. The star contracts to maintain virial equilibrium (Kelvin-Helmholz or KH contraction; phase III). The interior temperature rises during the contraction. Active hydrogen burning begins when the central temperature exceeds $10^7$ K. After that, the stellar radius increases following the mass-radius relation of main sequence stars (phase IV).

Case with Cold Disk Accretion {#ssec:d_acc}
-----------------------------

### Fiducial Model {#sssec:fid}

We now consider stellar evolution with cold disk accretion at the same rate $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$ (case MD3-D). First, we discuss the fiducial case with the $0.1~M_\odot$ initial model adopting $\beta = 1$ in equation (\[eq:s0\]). The top panel of Figure \[fig:struct\_log\_1em3b1\] shows the evolution of the stellar radius and interior structure. We see that the evolution differs from the spherical accretion case for $M_\ast \lesssim 10~M_\odot$, as previously demonstrated by YB08 (also see Appendix \[ap:cp\_yb\] for comparison to YB08). For $M_\ast \lesssim 5~M_\odot$ the stellar radius is much smaller than for spherical accretion. An outer convective zone appears in this phase. The protostar then abruptly inflates during the period $5~M_\odot \lesssim M_\ast \lesssim 9~M_\odot$. The maximum radius is $\simeq 90~R_\odot$ for $M_\ast \simeq 10~M_\odot$, which is comparable to the results of the spherical accretion case. The stellar radius decreases for $M_\ast \gtrsim 10~M_\odot$, and then finally follows the mass-radius relationship for main sequence stars when $M_\ast \gtrsim 30~M_\odot$. The evolution for $M_\ast \gtrsim 10~M_\odot$ is quite similar to what we discussed above for spherical accretion.

We define the following four phases based on the evolutionary features: (I) convection ($M_\ast \lesssim 5~M_\odot$), (II) swelling ($5~M_\odot \lesssim M_\ast \lesssim 9~M_\odot$), (III) KH contraction ($9~M_\odot \lesssim M_\ast \lesssim 30~M_\odot$), and (IV) main sequence accretion phase ($M_\ast \gtrsim 30~M_\odot$). The top panel of Figure \[fig:lev\_tsc\_1em3b1\_ph\] shows the evolution of the accretion timescale and KH timescale. We note that $t_{\rm KH}$ significantly decreases at $M_\ast \simeq 6~M_\odot$, when the protostar rapidly inflates. The timescale balance sharply changes from $t_{\rm acc} \ll t_{\rm KH}$ to $t_{\rm acc} > t_{\rm KH}$ here. As with spherical accretion, we attribute the sequence of the evolutionary phases from (I) to (III) to the inversion of the timescale balance. The lower panel of Figure \[fig:lev\_tsc\_1em3b1\_ph\] shows that this change is due to the rapid increase of stellar luminosity $L_\ast$ caused by the decrease of opacity in the stellar interior with increasing mass. The detailed evolution in each phase is explained below.

#### Convection Phase

The top panels of Figures \[fig:str\_log\_1em3b1\_sh\] and \[fig:struct\_log\_1em3b1\] show that the evolution at $M_\ast \lesssim 5~M_\odot$ is quite different between the spherical accretion case and disk accretion case. In the disk accretion case the protostellar radius is about one tenth of the value obtained for spherical accretion. This is explained by equation (\[eq:r\_entropy\]) and the fact that the entropy content within the star is much lower with disk accretion, a natural consequence of the different accretion geometry. With spherically symmetric accretion gas settles onto the star with high entropy generated in the accretion shock front. For cold disk accretion, on the other hand, the entropy of the accreting gas is reduced to the value in the stellar atmosphere by the gas’ ability to radiate into free space. Mass accretion hardly affects the average entropy in the stellar interior for the case of cold disk accretion. Equation (\[eq:r\_entropy\]) shows that the stellar radius decreases according to $R_\ast \propto M_\ast^{-1/3}$ in this case. We see this decrease for $M_\ast \lesssim 0.5~M_\odot$ in Figure \[fig:struct\_log\_1em3b1\].

Figure \[fig:struct\_log\_1em3b1\] shows that deuterium burning (D-burning) begins when $M_\ast \simeq 0.4~M_\odot$. This is in stark contrast to the spherical accretion case, where it begins much later ($M_\ast \simeq 6~M_\odot$), as shown in Figure \[fig:mr\_doff\]. This difference reflects the different evolution of the maximum temperature within the protostar $T_{\rm max}$ (middle panel of Fig. \[fig:struct\_log\_1em3b1\]). The early rise of $T_{\rm max}$ with disk accretion is explained by the relation, $$T = \frac{\mu}{\cal{R}} \frac{P}{\rho}
  \propto \frac{M_{\ast}}{R_{\ast}},
\label{eq:t_typ}$$ where $T$ is the typical temperature within the star ${\cal{R}}$ is the gas constant, and $\mu$ is the mean molecular weight. Equations (\[eq:typ\_rhop\]) were used again to derive the dependence on $M_\ast / R_\ast$. Equation (\[eq:t\_typ\]) means that, at the same stellar mass, the interior temperature is higher for the smaller stellar radius. Since the stellar radius $R_\ast$ is smaller for the disk accretion, the central temperature is higher for the same stellar mass. Thus, D-burning begins much earlier in the disk accretion case.

Figure \[fig:struct\_log\_1em3b1\] shows that convective zones emerge soon after deuterium burning begins. First, a convective zone appears near the center for $M_\ast \simeq 0.5~M_\odot$. However, this zone disappears soon, when available deuterium is exhausted. The D-burning layer moves to the outer part of the star, where fresh deuterium still remains. Another convective zone forms there, connecting the D-burning layer to the stellar surface, where newly accreted deuterium can be mixed down to the D-burning layer. When $M_\ast \gtrsim 1~M_\odot$ the total energy production rate by D-burning becomes nearly equal to the steady-state rate (bottom panel of Fig. \[fig:lev\_tsc\_1em3b1\_ph\]), $$L_{\rm D, st} \equiv \dot{M}_\ast \delta_{\rm D} =
                1500~L_{\odot} \left(
                               \frac{\dot{M}_\ast}{10^{-3}~M_{\odot}/{\rm yr}}
                             \right)
                             \left(
                               \frac{[ {\rm D/H} ]}{2.5 \times 10^{-5}}
                             \right),
\label{eq:l_dst}$$ where $\delta_{\rm D}$ is the energy available from the deuterium burning per unit gas mass.

For $M_\ast \gtrsim 1~M_\odot$, the radiative core extends outward and the outer convective layer with its D-burning shell becomes geometrically thinner. This evolution is a result of the decrease of opacity in the stellar interior; radiative heat transport becomes more efficient with the lower opacity. At the end of phase (I) convection ceases where the radiative heat transport is efficient enough to carry away the heat generated by deuterium burning. Fresh deuterium is no longer supplied to the D-burning layer which has now become radiative.

Figure \[fig:struct\_log\_1em3b1\] shows that the stellar radius gradually increases after the ignition of deuterium burning. This is because deuterium burning enhances the average entropy in the stellar interior. The surface convective layer absorbs the entropy generated by deuterium burning. Figure \[fig:sl\_1em3\_beta1\_ph\]-(I) clearly shows that the entropy in the surface convective layer rises with increasing stellar mass. The effect of deuterium burning is also seen in Figure \[fig:mr\_doff\], which depicts the evolution of the stellar radius when deuterium burning is artificially turned off at some point (dashed lines). We see that, if deuterium burning is turned off at $M_\ast = 3~M_\odot$, the stellar radius ceases to increase.

Figure \[fig:mr\_doff\] also presents the evolution via spherical accretion without deuterium burning (dashed line). We see that, unlike the case of disk accretion explained above, deuterium burning hardly affects the evolution. A key quantity to interpret this difference is the opacity when deuterium burning begins. With spherical accretion, deuterium burning begins late, when $M_\ast \simeq 6~M_\odot$ and the opacity within the star has already decreased sufficiently. The radiative heat transport is so efficient that the heat generated by deuterium burning is carried away before the convection arises. With disk accretion, on the other hand, the opacity is still high at the ignition of deuterium burning when $M_\ast \simeq 0.3~M_\odot$. Deuterium burning initiates the convection due to the inefficient radiative heat transport. In this case deuterium burning affects the stellar evolution until opacity becomes low enough owing to increasing the stellar mass.

#### Swelling Phase

The stellar radius rapidly increases in this phase. However, this is not a homologous expansion of the star. Only a small percent of the mass near the surface significantly bloats up. For $M_\ast \simeq 10~M_\odot$, for example, 10% of the total stellar mass fills 90% of the radius and 99.9% of the volume. Figure \[fig:struct\_log\_1em3b1\] also shows that the stellar interior structure changes during the swelling. The surface convective zone leaves the D-burning layer and moves outward for $M_\ast \simeq 6~M_\odot$. The radiative core covers most of the stellar interior.

What is the mechanism of the significant swelling? We contend that deuterium burning cannot be the primary cause, as demonstrated in the top panel of Figure \[fig:mr\_doff\]. We see that, even if we completely (artificially) turn off deuterium burning, the protostar subsequently inflates in all examined cases. Deuterium burning enhances the swelling, however; the earlier deuterium burning is turned off, the later the swelling occurs with a smaller maximum radius.

We examine the mechanism of the swelling by considering the evolution after turning off deuterium burning. Figure \[fig:slpf\_1em3\_ph\_doff4\] shows snapshots of entropy and luminosity profiles in each case. For $M_\ast \lesssim 8~M_\odot$ we find the characteristic feature of the “luminosity wave” in the luminosity profiles as in the spherical accretion case (see Section \[ssec:sp\_acc\], and Fig. \[fig:slpf\_1em3\_sh\]). The heat is transported from the interior where $\partial L / \partial M > 0$ to the surface layer where $\partial L / \partial M < 0$. The maximum luminosity increases with increasing stellar mass. At the same time the heat-losing interior extends outward toward the stellar surface. This characteristic evolution is caused by the decrease of opacity within the star. More and more entropy embedded in the deep stellar interior is transferred outward by radiation as the opacity decreases. The surface layer bloats up, because it has a high entropy through absorbing part of the transported entropy. Figure \[fig:slpf\_1em3\_ph\_doff4\] shows that the luminosity wave reaches the stellar surface for $M_\ast \simeq 9~M_\odot$. After that, $\partial L / \partial M > 0$ throughout the star and there is no entropy-receiving layer. However, the swelling still continues with disk accretion. This is because the newly accreted gas settles onto the star with the same high entropy of the stellar atmosphere. As a result, the surface layer always has high entropy. On the other hand, the stellar interior continues to lose entropy with decreasing opacity. The significant entropy loss in the stellar interior finally overcomes the swelling, and the star begins a phase of KH contraction.

Evolution of luminosity and entropy profiles with deuterium burning is shown in Figure \[fig:slpf\_1em3\_sh\]. The evolution is qualitatively similar to that without deuterium burning presented in Figure \[fig:slpf\_1em3\_ph\_doff4\]. Deuterium burning increases the entropy within the star, which makes the heat transport after the opacity decreases more significant. Therefore, deuterium burning enhances the swelling. Figure \[fig:slpf\_1em3\_sh\] shows that with deuterium burning the luminosity wave reaches the surface when $M_\ast \simeq 6~M_\odot$. The stellar surface luminosity $L_\ast$ significantly increases at this moment, which causes the inversion of the timescale balance (Fig. \[fig:lev\_tsc\_1em3b1\_ph\]).

#### Later Phases

For $M_\ast \gtrsim 9~M_\odot$ the protostar begins to contract ($t_{\rm KH} < t_{\rm acc}$). The protostar efficiently loses its energy by radiation. Figure \[fig:sl\_1em3\_beta1\_ph\] shows that the entropy in the stellar interior decreases during this phase. The maximum temperature within the star soon exceeds $10^7$ K. Hydrogen burning begins first via the pp-chain followed by CNO-cycle reactions, which lead to a convective core emerges when $M_\ast \simeq 20~M_\odot$. The stellar surface luminosity becomes nearly equal to the total energy production rate by CNO-cycle hydrogen burning for $M_\ast \simeq 30~M_\odot$ (Fig. \[fig:lev\_tsc\_1em3b1\_ph\]). The stellar mass when the protostar reaches the ZAMS $M_{\ast, {\rm ZAMS}}$ is analytically estimated by equating the accretion timescale to the KH timescale of ZAMS stars: $$t_{\rm acc} \simeq t_{\rm KH,ZAMS} .
\label{eq:t_mzams}$$ For $10~M_\odot \lesssim M_\ast \lesssim 100~M_\odot$ the mass-radius and mass-luminosity relationships of ZAMS stars (e.g. Schaller et al. 1992) are well fitted by: $$L_{\ast, {\rm ZAMS}} = 1.4 \times 10^4~L_\odot
\left( \frac{M_\ast}{10~M_\odot} \right)^2 ,
\label{eq:l_zams}$$ $$R_{\ast, {\rm ZAMS}} = 3.9~R_\odot
\left( \frac{M_\ast}{10~M_\odot} \right)^{0.55} .
\label{eq:r_zams}$$ Substituting these relations into equation (\[eq:t\_mzams\]), we get $$M_{\ast, {\rm ZAMS}} \simeq 30.5~M_\odot
\left( \frac{\dot{M}_\ast}{10^{-3}~M_{\odot}~{\rm yr}^{-1}}
\right)^{0.645} ,
\label{eq:mzams}$$ which agrees well with our calculations. Since the above argument is independent of different accretion geometries, so is $M_{\ast, {\rm ZAMS}}$.

### Dependence on Initial Models {#sssec:imod}

Next, we examine how the protostellar evolution changes with different initial models. To this end we consider two initial models that differ from the the fiducial one. One is a $0.1~M_\odot$ star with a shallower initial entropy distribution ($\beta = 0.1$ in equation (\[eq:s0\]); case MD3-D-b0.1). The other is a fully convective $1.3~M_\odot$ star (case MD3-D-cv), which was used by Palla & Stahler (1992) to calculate the evolution at $\dot{M}_\ast = 10^{-4}~M_{\odot}~{\rm yr}^{-1}$ via cold disk accretion. Figure \[fig:1em3\_ph\_ini\] shows the evolution of stellar radius and maximum temperature in these cases. The basic evolution is similar. A protostar undergoes swelling and contraction, finally reaching the main sequence accretion phase when $M_\ast \simeq 30~M_\odot$. However, the evolution differs quantitatively for the different initial models. For example the maximum stellar radius is $\simeq 400~R_\odot$ for case MD3-D-b0.1, but $\simeq 30_\odot$ for case MD3-D-cv (the evolution of the interior structure in these cases also differs slightly from that for case MD3-D described in Section \[ssec:d\_acc\]; see Appendix \[ap:b0.1\] for details).

This is in stark contrast to the spherical accretion case, where the evolution is almost independent of different initial models. For spherically symmetric accretion the evolution of stellar radius in the adiabatic accretion phase is well approximated by the relation (Stahler, Palla & Salpeter 1986): $$R_{\ast} \simeq  26~R_{\odot} \left( \frac{M_{\ast}}{M_{\odot}} \right)^{0.27}
                 \left( \frac{\dot{M}_\ast}
                             {10^{-3}~M_{\odot}~{\rm yr}^{-1}} \right)^{0.41}.
\label{eq:r_sps86}$$ Our calculated evolution with spherical accretion (case MD3-S) also obeys this relation before the swelling occurs. Stahler, Palla & Salpeter (1986) showed that the evolution of the radius converges to the above relation even beginning with different initial models. With spherical accretion entropy generated at an accretion shock front is taken into the stellar interior along with the accreted gas. If the initial radius is too large compared to equation (\[eq:r\_sps86\]), the accretion shock front is weak due to the shallow gravitational potential well. The entropy produced at the accretion shock front is reduced, which decreases average entropy within the star. As a result the protostar contracts. If the initial radius is too small, the opposite occurs, increasing the radius. With disk accretion, however, this regulation process does not operate. The entropy of the accreted material is set to the value in the stellar atmosphere. Since the structure of the stellar atmosphere differs with different initial models, the subsequent evolution also changes (also see Hartmann et al. 1997 for low-mass protostars).

How should we choose the initial model? We infer this by considering the evolution of accretion flow toward the protostar. Just after a protostar is born, the protostar gathers material from its immediate vicinity with low angular momentum. The geometry of the accretion flow is nearly spherical in this early phase. Afterwards, gas originally far from the star falls toward the star with increasingly higher angular momentum. A circumstellar disk forms, and the protostar continues to grow via disk accretion. The protostellar evolution in this scenario is calculated by switching the accretion geometry from spherical to disk accretion at some point.

Figure \[fig:m\_rsh\] shows some examples of protostellar evolution, whereby the accretion geometry is switched for $M_\ast = 0.1~M_\odot$ and $1~M_\odot$. The protostellar radius increases in the early spherical accretion phase according to equation (\[eq:r\_sps86\]). The radius subsequently decreases after the geometry is switched to cold disk accretion, because the accreting gas brings lower entropy into the stellar interior. The interior temperature increases as the protostar contracts. Active deuterium burning begins when the maximum temperature exceeds $\simeq 10^6$ K. Figure \[fig:m\_rsh\] shows that, the earlier the geometry is switched, the earlier deuterium burning begins. The subsequent evolution is similar to that in our fiducial case MD3-D explained in Section \[ssec:d\_acc\]. The maximum radius is $\simeq 50~R_\odot$ in both examined cases. The protostar reaches the main sequence accretion phase at $M_\ast \simeq 30~M_\odot$, which is independent of the history of accretion geometry.

Comparison with Primordial Protostars {#ssec:metal}
-------------------------------------

Rapid mass accretion $\dot{M}_\ast \sim 10^{-3}~M_{\odot}~{\rm yr}^{-1}$ is also expected during the formation of primordial ($Z = 0$) stars. Here, we compare the evolution of primordial protostars to that of present-day ($Z = Z_\odot$) massive protostars. Figure \[fig:m\_rz\] presents the evolution of the stellar radius with metallicities $Z = 0$ (case MD3-SDm0.1-z0) and $Z = Z_\odot$ (case MD3-SDm0.1). In these cases the accretion geometry is switched from spherical accretion to disk accretion at $M_\ast = 0.1~M_\odot$. The basic evolution with $Z = 0$ is the same as in the present-day case. After deuterium burning begins for $M_\ast \simeq 0.8~M_\odot$, the protostar undergoes the four evolutionary phases of convection, swelling, KH contraction, and main sequence accretion.

However, Figure \[fig:m\_rz\] also shows some quantitative differences between the primordial and present-day cases. At $Z = 0$, for example, the swelling occurs for $M_\ast \simeq 6~M_\odot$, which is slightly earlier than for solar metalicities. A similar difference is also found with spherical accretion, as shown in Figure \[fig:m\_rz\]. These differences are attributed to the fact that the opacity is lower at lower metallicity in the same thermal state. As explained in Section \[ssec:sp\_acc\] and \[ssec:d\_acc\], the swelling occurs as a result of the decrease of opacity in the stellar interior with increasing the stellar mass. The swelling occurs earlier at $Z=0$, because the opacity decreases sufficiently at an earlier time.

Another difference between the primordial and present-day case is the stellar radius in the main sequence accretion phase; the ZAMS radius for $Z=0$ is much smaller than that for $Z = Z_\odot$, independent of the assumed geometry. In the primordial case the initial abundance of C, N, and O nuclei, necessary catalysts for the CNO-cycle hydrogen burning, is zero. CNO-cycle reactions do not begin until these atoms are provided by helium triple-$\alpha$ burning, which occurs at $T \simeq 10^8$ K. Because pp-chain hydrogen burning does not supply sufficient energy to halt the star’s KH contraction, the pre-main contraction phase continues up to the higher central densities and temperatures that allow triple-$\alpha$ reactions. This ZAMS star thus has a much smaller radius than its solar metallicity counterpart.

Dependence on Mass Accretion Rates {#sec:mdot_dep}
==================================

Finally, we examine how the protostellar evolution changes with different accretion rates. As pointed out in Section \[sssec:imod\], the evolution quantitatively varies with different initial models even at the same accretion rate. In this section we focus on the cases where the accretion geometry evolves from spherical accretion to disk accretion in early phases. Figure \[fig:m\_r\_mdotv\] displays the evolution of the stellar radius at the accretion rates of $\dot{M}_\ast = 10^{-4}~M_{\odot}~{\rm yr}^{-1}$ (case MD4-SDm0.1), $10^{-3}~M_{\odot}~{\rm yr}^{-1}$ (case MD3-SDm0.1), and $4 \times 10^{-3}~M_{\odot}~{\rm yr}^{-1}$ (case MD4x3-SDm0.5). With the rate $10^{-4}~M_{\odot}~{\rm yr}^{-1}$, the protostar undergoes the same four evolutionary phases as with the rate $10^{-3}~M_{\odot}~{\rm yr}^{-1}$. The maximum radius decreases with decreasing the accretion rate. The same dependence is also seen with spherical accretion. Note that, however, the maximum radius varies with different initial models under the assumption of a freely radiating photospheric boundary (“disk accretion”) as explained in Section \[sssec:imod\]. Figure \[fig:m\_r\_mdotv\] also shows that, at lower accretion rates, the protostar arrives to the main-sequence accretion phase at a lower stellar mass. We argue that this dependence is robust. The stellar mass at the arrival to the ZAMS is just determined by $t_{\rm acc} \simeq t_{\rm KH, ZAMS}$ as shown by equation (\[eq:mzams\]), which is independent of different accretion geometries and different initial models.

Figure \[fig:m\_r\_mdotv\] shows a qualitatively different evolution at the higher rate $\dot{M}_\ast = 4 \times 10^{-3}~M_{\odot}~{\rm yr}^{-1}$. With spherical accretion a period of rapid expansion occurs when $M_\ast \simeq 50~M_\odot$. This expansion was originally found by Omukai & Palla (2001, 2003) at zero metallicity. The expansion occurs when the total luminosity $L_{\rm tot}$ approaches the Eddington luminosity, where $L_{\rm tot} = L_\ast + L_{\rm acc}$ and $L_{\rm acc}$ is an additional component from the accretion shock front, $L_{\rm acc} = G M_\ast \dot{M}_\ast / R_\ast$. In Paper I, we showed that the critical Eddington ratio $L_{\rm tot}/L_{\rm Edd}$, above which the expansion occurs, is about 0.5 at $Z=Z_\odot$ (presented again in Figure \[fig:ledd\]). The critical ratio less than unity is because the opacity near the stellar surface is somewhat higher than the electron-scattering opacity.

When $L_{\rm tot}$ reaches $0.5 L_{\rm Edd}$ in the KH contraction phase, rapid expansion occurs and inhibits growth of the protostar by steady mass accretion. We can derive the critical accretion rate $\dot{M}_{\rm \ast, cr}$, with which the protostar barely reaches the ZAMS without undergoing rapid expansion, from the critical Eddington ratio as follows (Omukai & Palla 2003; Paper I). In the critical case, $L_{\rm tot}$ reaches $0.5 L_{\rm Edd}$ when the protostar arrives to the ZAMS. Thus, in the spherical accretion case, the critical rate $\dot{M}_{\rm \ast,cr}$ satisfies the relation $$L_{\rm ZAMS} + \frac{G M_{\rm ZAMS} \dot{M}_{\rm \ast,cr}}{R_{\rm ZAMS}}
= 0.5 L_{\rm Edd} ,$$ where the suffix “ZAMS” indicates the quantities of ZAMS stars. This relation is transformed to $$\dot{M}_{\rm \ast,cr} = \frac{4 \pi c R_{\rm ZAMS}}{\kappa_{\rm esc}}
              \left( 1 - \frac{L_{\rm ZAMS}}{0.5 L_{\rm Edd}} \right) ,$$ where $\kappa_{\rm esc}$ is the electron-scattering opacity, a lower limit to the actual opacity. The critical rate given by this equation is a function of $M_\ast$, but its dependence is weak. The numerical value is $\dot{M}_{\rm \ast,cr} \simeq
3 \times 10^{-3}~M_\odot~{\rm yr}^{-1}$ over a wide range of $M_\ast$, which is consistent with our numerical results.

We see that a similar expansion also occurs for $4 \times 10^{-3}~M_{\odot}~{\rm yr}^{-1}$ in the cold disk accretion limit in Figure \[fig:m\_r\_mdotv\]. In this case the protostar very abruptly inflates when $M_\ast \gtrsim 20~M_\odot$ and never turns to KH contraction. The stellar radius finally exceeds $600~R_\odot$ for $M_\ast \simeq 30~M_\odot$. YB08 also reported a similar evolution for the accretion rate $10^{-2}~M_{\odot}~{\rm yr}^{-1}$. Interestingly, it is known that a similar expansion also occurs when a main-sequence star undergoes rapid mass accretion due to mass exchange in close binary systems. Kippenhahn & Mayer-Hofmeister (1977) and Neo et al. (1977) considered the accretion of deuterium-free gas onto existing main sequence stars. The numerical method they adopted is basically the same as ours; the protostellar structure was numerically calculated with a freely radiating photospheric boundary condition.

Figure \[fig:ledd\] shows that the critical Eddington ratio for the expansion is also $L_\ast / L_{\rm Edd} \simeq 0.5$ in the cold disk accretion limit. Note that there is no additional luminosity component $L_{\rm acc}$ here. The accretion luminosity is assumed to have already radiated into free space before the accreted material settles onto the star. The critical accretion rate in this case is derived as follows. As explained in Section \[ssec:d\_acc\], the stellar luminosity $L_\ast$ significantly rises in the swelling phase. The luminosity comes from release of gravitational energy after that. Figure \[fig:ledd\] shows that the stellar luminosity in this phase roughly follows $$L_\ast \simeq 3 \times L_{\rm ZAMS} (M_\ast)
\label{eq:lst}$$ in all cases considered. The stellar luminosity approaches $L_{\rm ZAMS} (M_\ast)$ just before the arrival to the ZAMS at the rate $10^{-4}$ and $10^{-3}~M_\odot~{\rm yr}^{-1}$. At the rate $4 \times 10^{-3}~M_\odot~{\rm yr}^{-1}$, however, $L_\ast$ approaches $0.5 L_{\rm Edd}$ before reaching the ZAMS and the abrupt expansion occurs. The stellar mass at which $L_\ast \simeq 0.5 L_{\rm Edd}$ is $M_\ast \simeq 45~M_\odot$ using equation (\[eq:lst\]). In order to avoid expansion the protostar has to reach the ZAMS with a mass $M_{\rm \ast, ZAMS} \lesssim 45~M_\odot$. This condition is transformed to that for accretion rates with equation (\[eq:mzams\]), $$\dot{M} \lesssim \dot{M}_{\rm \ast, cr}
\simeq 2 \times 10^{-3}~M_\odot~{\rm yr}^{-1} .$$ The derived critical rate is comparable to that for spherically symmetric accretion, as confirmed by our numerical calculations.

Our calculations suggest that a massive protostar significantly bloats up and can not reach the ZAMS by steady mass accretion, if the accretion rate is higher than a few $10^{-3}~M_\odot~{\rm yr}^{-1}$. This feature is independent of the accretion geometry. If mass accretion completely shuts off as a result of the fast expansion of the protostar, there will be an upper mass limit of pre-main-sequence stars around several 10s$~M_\odot$, as discussed in Paper I. Otherwise, mass accretion might continue in a non-steady fashion. At least, it is certain that the radius of a massive protostar reaches several 100s$~R_\odot$ at the high accretion rate. The very large radius leads to a low effective temperature of the protostar.

For case MD4x3-SDm0.5, for example, the stellar luminosity exceeds $10^5~L_\odot$ for $M_\ast \gtrsim 18~M_\odot$, but the effective temperature is only $T_{\rm eff} \lesssim 10^4$ K, the value of a $M_\ast \lesssim 2.5~M_\odot$ ZAMS star. The stellar UV luminosity is very low for such low $T_{\rm eff}$. This is important for the growth of an H II region around the protostar (e.g., Hoare & Franco 2007). Observationally, High-Mass Protostellar Objects (HMPOs) are considered to be young forming massive stars prior to the formation of an H II region. However, a lot of HMPOs have high infrared luminosity exceeding $10^4~L_\odot$ without observable H II regions (e.g., Sridharan et al. 2002; Beltrán et al. 2006b; Beuther et al. 2007). There has been some speculation regarding what hinders the growth of H II regions around these bright sources. ZAMS stars with such high luminosity should ionize their surroundings. Some authors have proposed that rapid mass accretion quenches the growth of H II regions by increasing the gas density and recombination rate near the protostar (e.g., Walmsley 1995). With disk accretion, however, the H II region would breaks out in the polar direction, where the gas density decreases significantly after the material with low angular momentum has accreted onto the star or been expelled in an outflow.

Our calculations well explain the existence of such bright HMPOs even with disk accretion. Massive stars accreting at high rates bloat up; their UV luminosity is too low to form the H II region.

Summary and Conclusions {#sec:sum}
=======================

In this paper we have studied the evolution of massive protostars with disk accretion at high rates $\dot{M}_\ast > 10^{-4}~M_{\odot}~{\rm yr}^{-1}$. We considered the limiting case of “cold” disk accretion, whereby most of the stellar surface is not affected by the accretion flow, and the accreting material brings a minimum of entropy into the star. We calculated the evolution of protostars in this limiting case by adopting the photospheric (freely radiating) boundary condition. The calculated evolution was compared and contrasted to the evolution with spherically symmetric accretion, corresponding to the opposite limit, whereby the accreting gas transports the maximum amount of entropy into the star.

First, we considered in detail the evolution for $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$. The basic evolution via the cold disk accretion is summarized as follows:

The entire evolution is divided into four evolutionary phases: (I) convection, (II) swelling, (III) KH contraction, and (IV) the main-sequence accretion phase. The evolution in the first three phases varies with different initial models. Roughly speaking, the stellar radius reaches its maximum $30 - 400~R_\odot$ for $M_\ast \simeq 10~M_\odot$ at the end of the swelling phase (II). On the other hand, the protostar begins the final phase (IV) for $M_\ast \simeq 30~M_\odot$, independent of different initial models.

A key physical quantity governing the evolution is the opacity in the stellar interior, analogous to the spherical accretion case. The opacity decreases with increasing stellar mass, which causes the variety of the evolution. In phase (I) the opacity is so high that the radiative heat transport within the star does not affect the stellar structure. In phase (II) the entropy accumulated in the stellar interior is gradually transported outward as the opacity decreases. A part of the transported entropy is received in a thin layer near the stellar surface. Due to the high entropy deposited into this layer it significantly bloats up, resulting in the swelling seen in phase (II). Afterwards, the opacity decreases sufficiently, allowing the star to lose heat by efficiently radiation. The protostar contracts and the interior densities and temperatures rise. This is the KH contraction phase (III). The protostar finally reaches the main-sequence accretion phase (IV), just after the active hydrogen burning begins.

A major difference between the results for spherical accretion and cold disk accretion is the role of deuterium burning. In the limit of cold disk accretion the accreting gas brings a minimal amount of entropy into the star. Since the stellar radius is smaller because of the lower average entropy in the stellar interior, the protostellar radius is initially small, $R_\ast \simeq$ a few $\times R_\odot$. However, deuterium burning begins earlier, which raises the entropy content within the star. This enhances the swelling. Consequently, the maximum radius is as large as that with spherical accretion.

Next, we calculated the protostellar evolution at zero metallicity in the cold disk accretion limit. The protostellar evolution varies with metallicities in the same manner as with spherical accretion; at $Z = 0$, the protostar swells up slightly earlier, and reaches the ZAMS with a smaller stellar radius.

Finally, we examined the evolution with different accretion rates. Our calculations show some dependences on accretion rates which were also found with spherical accretion. First, the stellar mass at the arrival to the ZAMS is higher for higher accretion rates. However, if the accretion rate is higher than a few $10^{-3}~M_\odot~{\rm yr}^{-1}$, the stellar radius continues to increase without returning to KH contraction. The protostar never reaches the ZAMS by steady mass accretion at such high rates.

The fact that a massive protostar bloats up to a radius of several 100s$~R_\odot$ with an accretion rate exceeding $10^{-3}~M_\odot~{\rm yr}^{-1}$ is a very robust result of our studies. The large radius leads to a low effective temperature and a correspondingly low stellar UV luminosity. Thus, the growth of an H II region will be delayed until mass accretion onto the star deceases significantly. This explains the existence of HMPOs with high luminosities exceeding $10^4~L_\odot$.

[ We thank Peter Bodenheimer for a careful critique of the manuscript. We also thank Neal Turner for fruitful comments and discussions. This study is supported in part by Research Fellowships of the Japan Society for the Promotion of Science for Young Scientists (TH) and by the Grants-in-Aid by the Ministry of Education, Science and Culture of Japan (18740117, 18026008, 19047004: KO). Portions of this work were conducted at the Jet Propulsion Laboratory, California Institute of Technology, operating under a contract with the National Aeronautics and Space Administration (NASA). ]{}

Evolution for $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$ with Shallow Initial Entropy Profile {#ap:b0.1}
===================================================================================================

In Section \[sssec:imod\], we have seen that the protostellar evolution differs with different initial models under the cold disk accretion even at the same accretion rate. In this appendix, we add a more detailed explanation of these differences. We revisit case MD3-D-b0.1 (Section \[sssec:imod\]), whereby the initial entropy distribution is shallower than for the fiducial case MD3-D. The principle difference occurs in the first convection phase (I) (see Figure \[fig:str\_log\_1em3b0.1\]). A central convective core emerges soon after the onset of deuterium burning when $M_\ast \simeq 0.3~M_\odot$. The convective core grows outward and merges with the outer convective layer near the surface: The protostar becomes fully convective for $M_\ast \simeq 0.4~M_\odot$. This is not seen in case MD3-D, where the core remains radiative even after D-burning begins.

The subsequent evolution also differs. For case MD3-D (see Figure \[fig:struct\_log\_1em3b1\]) the radiative core gradually extends outward with increasing the stellar mass. The D-burning layer, located at the bottom of the outer convective layer, also moves outward, until the protostar swells up ($M_\ast \simeq 6~M_\odot$). For case MD3-D-b0.1, on the other hand, deuterium burning continues at the stellar center as long as the protostar remains fully convective and freshly accreted gas (containing deuterium) is mixed downward. The deuterium is significantly depleted in this fully convective phase (lower panel of Fig. \[fig:str\_log\_1em3b0.1\]). When $M_\ast \simeq 5~M_\odot$ a thin radiative layer (a so-called “radiative barrier”) forms within the star, and the stellar structure changes significantly. This radiative barrier blocks the convective transport of newly accreted deuterium into the stellar interior. Without the refurbishment of deuterium, the central zones quickly consume all available deuterium and become radiative. Deuterium burning continues in a thin layer outside the radiative core.

The evolution described above is simlar to that of intermediate-mass protostars as calculated by Palla & Stahler (1991, 1992; also see Appendix \[ap:cp\_ps\] below). The significant heat input by the deuterium shell-burning triggers the rapid swelling of the star. The stellar radius ultimately expands to about $400~R_\odot$. As in case MD3-D, however, deuterium shell-burning per se is not the main driver of the swelling. Figure \[fig:str\_log\_1em3b0.1\] shows that, even if we turn off D-burning just after the swelling begins, the protostar continues to swell up. The protostar expands because a thin surface layer bloats up after receiving entropy transported from the inner part of the star.

Comparison with Previous Work {#ap:prev}
=============================

Comparison with Palla & Stahler (1992) {#ap:cp_ps}
--------------------------------------

We compare our numerical results with previous calculations by Palla & Stahler (1992), who studied protostellar evolution in the limit of cold disk accretion with accretion rates $10^{-5}~M_{\odot}~{\rm yr}^{-1}$ and $10^{-4}~M_{\odot}~{\rm yr}^{-1}$. The numerical method adopted by Palla & Stahler (1992) is the same as ours (e.g., Stahler, Shu & Taam 1980). The same photospheric boundary condition (equations \[eq:psb\_p\] and \[eq:psb\_l\]) was used for the limiting case of cold disk accretion. The initial models they adopted are $1.0~M_\odot$ and $1.3~M_\odot$ fully convective stars at accretion rates of $10^{-5}~M_{\odot}~{\rm yr}^{-1}$ and $10^{-4}~M_{\odot}~{\rm yr}^{-1}$, respectively. We also constructed the same initial models following their method and calculated the subsequent evolution at each accretion rate. Figure \[fig:m\_r\_ps\] shows the resulting mass-radius relations. Our calculations agree well with the results presented by Palla & Stahler (1992). For these cases the protostar remains fully convective until just before the swelling, when a radiative barrier appears as for case MD3-D-b0.1 discussed above.

In section \[sec:mdot\_dep\] we discussed another case with $10^{-4}~M_{\odot}~{\rm yr}^{-1}$ (case MD4-SDm0.1) in addition to that shown in Figure \[fig:m\_r\_ps\]. Because the initial models differ, the mass-radius relations are slightly different between these cases, although the adopted accretion rate and boundary condition are the same.

Comparison with Yorke & Bodenheimer (2008) {#ap:cp_yb}
------------------------------------------

Next, we compare the results presented in Section \[ssec:d\_acc\] to the previous calculations by YB08 (see also discussion in Section \[sec:intro\]). YB08 independently calculated the evolution of accreting massive protostars by solving the interior structure using a different numerical code than that used by Palla & Stahler (1992). To make the comparison clear we recalculate the evolution with their code and briefly analyze the evolution of the stellar interior structure. The basic equations are the usual four stellar structure equations, taking into account the effect of mass accretion. The adopted boundary condition slightly differs from the one depicted in equations (\[eq:psb\_p\]) and (\[eq:psb\_l\]), but is essentially the same photospheric boundary condition (Bodenheimer et al. 2007; YB08). YB08 solve for a spherical grey stellar atmosphere including curvature effects. The stellar interior models are constructed using the Henyey method iterated to match the grey atmosphere. The initial model is a fully convective $0.1~M_\odot$ star of radius $1~R_\odot$.

Figure \[fig:struct\_log\_yb\] shows the evolution of the stellar radius and interior structure for $\dot{M}_\ast = 10^{-3}~M_{\odot}~{\rm yr}^{-1}$. The protostar is initially fully convective, until a radiative core appears for $M_\ast \simeq 0.8~M_\odot$. The subsequent evolution is very similar to that for case MD3-D discussed in Section \[sssec:fid\] (see Fig. \[fig:struct\_log\_1em3b1\] for comparison). The radiative core gradually grows outward as the stellar mass increases. The D-burning layer, located at the bottom of the outer convective layer, also moves outward. The stellar radius remains $\sim 1~R_\odot$ during this phase, which is slightly smaller than for case MD3-D. At this smaller radius (and higher central densities and temperatures) central hydrogen burning occurs earlier than for case MD3-D. The protostar rapidly swells up when $M_\ast \simeq 4~M_\odot$. The radiative core simultaneously expands to cover most of the star. Central hydrogen burning nearly dies out.

As noted in Section \[sssec:fid\], deuterium burning itself is not the cause of the swelling. Figure \[fig:struct\_log\_yb\] shows that even if all nuclear reactions are turned off when $M_\ast \simeq 3.5~M_\odot$, the protostar significantly swells up later. After the stellar radius reaches its maximum of $120~R_\odot$ when $M_\ast \simeq 13~M_\odot$, the protostar contracts and hydrogen burning increases in the center. The convective core also grows due to the increased heat input by hydrogen burning. The star reaches the ZAMS for $M_\ast \simeq 30~M_\odot$ and continues to closely follow the ZAMS as it accretes new material. All these evolutionary features are also seen in case MD3-D. We conclude that the evolution presented in Section \[ssec:d\_acc\] is fully consistent with the previous calculation by YB08.


In the context of the present invention, a prosthesis is a manufactured device for replacing a missing part of a body, such as a limb or portion thereof. There are two basic types of prosthesis: exoskeletal and endoskeletal. An exoskeletal prosthesis, also called a crustacial prosthesis, is supported by a rigid outer shell. An endoskeletal prosthesis is supported by internal support members. That is, structural support is provided by members inside the prosthesis.
Endoskeletal protheses are rapidly growing in popularity. A need exists for a reliable and efficient device and method that does not require a high degree of specialized equipment and/or skill for attaching an endoskeletal prosthesis to a patient, such as to the patient's molded stump socket or bandage wrap stump socket.
A stump socket is typically made by molding material around a person's stump or a positive model of the stump thereby forming a prosthetic socket or stump socket that can be worn by a patient over the stump and a remaining portion of a person's limb. Once the socket has been manufactured, or while it is being manufactured, it is secured to an attachment device which is then mounted to the endoskeletal prosthesis, typically by molding a portion of the stump socket to the attachment device.
A bandage wrap stump socket is made by applying activated plaster or resin bandage material over a person's stump and adjacent residual limb after an amputation operation.
Two types of attachment devices are known in the prior art. One type of attachment device that is commonly utilized to mount the stump socket to the prosthesis, shown in FIG. 3, is a flat metal disc or plate 30, typically having four threaded holes. The metal disc or plate can be round or square. Typically, the prosthesis is bolted or secured by other suitable threaded fasteners to the coupler thereby providing an artificial limb for the patient to wear. In order for the metal disc to be more securely attached to the stump socket, thermoplastic or other suitable material is molded around the periphery of the metal plate and around the bottom side of the metal plate opposite the side at which the persons' stump is to be located. Otherwise, the socket would detach more easily during use especially if a thermoforming resin is used. Thermoforming resins, such as polypropylene are especially difficult to use because such resins shrink when cooled. This bottom side is the same side to which the prosthetic device attaches to the plate by means of threaded fasteners. Thus, there is a layer of thermoplastic material between the plate and the end of the prosthetic device through which the fasteners pass to secure the prosthetic device to the plate. Since plastic material is sandwiched between the metal attachment plate and portion of the prosthesis attached to the plate, which is usually also metal, the plastic typically will deform under load and ,causes the socket to become loose. Some metal plate attachment devices have knurls on their side surfaces to facilitate attachment of the plate to the thermoplastic of the socket, but it is still necessary for the thermoplastic to be formed around the bottom side of the plate.
The flat metal plate attachment device poses an additional problem. During fitting to a patient, it is difficult to locate the metal plate on either the stump or on a positive model of the stump in the desired orientation. Since stumps and therefore the stump models typically have rounded ends, the flat metal plate device must be maintained in the desired orientation on the rounded end of the stump and/or stump model during the placing and at least partial curing of the moldable material around the metal plate and the socket. This balancing of the metal plate device is difficult, time consuming and skill intensive.
The second known attachment device is a wood attachment block 27, illustrated in FIG. 4. In order to fit the block to a patient, top surface 28 of wooden block 27 is carved out to fit the contours of the patient's stump socket. Typically, this requires a high level of skill and is time intensive. In addition, to secure the contoured wood block to the stump socket, thermosetting resins are typically used for the required adhesion to wood. These resins are difficult to work with because they are generally liquid and also are time consuming and toxic. Thus, not only is the fitting of wooden attachment blocks skill and time intensive, but it typically requires the use of toxic material to attach the block to the stump socket. Thermoforming resins are generally not suitable for wood attachment blocks.
Therefore, a need exists for a prosthetic attachment device that securely attaches to a prosthetic socket or stump socket without the aforementioned limitations. In addition, a need exists to reduce the amount of time and skill needed to attach an endoskeletal prosthesis to a prosthetic or stump socket. A need exists that permits use of thermoforming resins (especially polypropylene and transparent resins) without extending the resin over the bottom of the attachment device.


/*
 * Copyright (c) 2012-2014, Parallel Universe Software Co. All rights reserved.
 *
 * This program and the accompanying materials are dual-licensed under
 * either the terms of the Eclipse Public License v1.0 as published by
 * the Eclipse Foundation
 *
 *   or (per the licensee's choosing)
 *
 * under the terms of the GNU Lesser General Public License version 3.0
 * as published by the Free Software Foundation.
 */
package co.paralleluniverse.common.collection;

import it.unimi.dsi.fastutil.longs.AbstractLongCollection;
import it.unimi.dsi.fastutil.longs.AbstractLongIterator;
import it.unimi.dsi.fastutil.longs.LongIterator;

/**
 *
 * @author pron
 */
public class LongRange extends AbstractLongCollection {
    final long start;
    final int length;

    public LongRange(long start, int length) {
        this.start = start;
        this.length = length;
    }

    @Override
    public int size() {
        return length;
    }

    @Override
    public LongIterator iterator() {
        return new AbstractLongIterator() {
            private int nextIndex = 0;

            @Override
            public boolean hasNext() {
                return nextIndex < length;
            }

            @Override
            public long nextLong() {
                return start + (nextIndex++);
            }

            @Override
            public void remove() {
                throw new UnsupportedOperationException();
            }
        };
    }

    @Override
    public boolean contains(long entry) {
        return (entry >= start && entry < (start + length));
    }

    @Override
    public boolean rem(long entry) {
        throw new UnsupportedOperationException();
    }

    @Override
    public void clear() {
        throw new UnsupportedOperationException();
    }
}


  {$comment.Author.Name}{$comment.Time()} | {$lang['Zit']['reply']}
  <q>{$comment.Content}</q>
  {foreach $comment.Comments as $comment}
  {template:comment}
  {/foreach}


The Open SD-Access Network: Why Now?

As a number of factors converge to herald a new software defined shift, and with SD access becoming mainstream, software defined networks (SDN) and network function virtualization (NFV) are increasingly working their way into the wider communications discussion.

But what does it mean for service providers? Why is now the right time to embrace it?

While the terms SDN and NFV are bandied around, the lack of industry education around them poses a potential barrier when trying to link the potential of this new technology and the way we do business more widely.

What this means for how we do business

As the world becomes increasingly digital, it’s impossible to ignore how SD access might influence a large-scale shift to a much more inclusive, flexible and fair way of doing business.

The open architecture of SD access creates a less complex environment in which information can be utilized to create novel applications much more quickly. Its malleable, open source nature makes it interoperable, giving you the flexibility to bolt anything on, big or small, which in turn creates an inclusive digital landscape that allows the offerings of smaller, nimbler start-ups to rub along with the digital giants of the era.

This network flexibility and capability renders new possibilities for providers, working with cloud-based products to provide value-added offerings - which they can monetize. They can classify traffic types on the network in real-time, and make decisions about how the different traffic types are handled across the network. They can offer providers of cloud-based services to whom latency and packet-loss are very important, for example, an SLA (service level agreement) which guarantees their customers an enhanced online experience and boosts the power of their cloud-based offering.

The role of the network provider is shifting from ‘dumb pipe’ to ‘services provider’, with value-added services, which can optimize the offering a service provider takes to their customers. Instead of the incumbent pipeline model, which looks towards and tries to monetize everything from the consumer, networks such as these lead to a two-sided interaction between network and service providers - which better lends itself to a platform-based economy.

As business becomes increasingly digitized, and dependence on the cloud accelerates daily, the transparent, horizontal transactions in environments such as the software defined network provide a great opportunity to start-up service providers, who can go straight to network providers for enhanced services; and the chance for smaller, nimbler network providers to enhance their offering and ultimately add significant value to their business.

Why now?

Regulators have noticed the potential benefits of this shift to business, and are either responding by softening their stance, or keeping their ears to the ground.

At the FTTH Conference in February, the EU Commission’s director of electronic communication networks and services, Anthony Whelan, recognized publicly that while net neutrality rules were put in place for good reason, the potential to pose an obstacle to service innovation exists, and clarified that although they want to protect against the negative discrimination of OTT services, not at the expense of service providers’ ability to expedite new and improved services. He added that if providers are in breach (i.e. negatively discriminating against other traffic flows), they’ll have to answer to the Commission, but over and above that, they’ll be allowed to apply a higher QoS as they deem fit for different traffic flows.

Of course, EU Commission rules don’t automatically extend to regional territories, and for the UK there is the added uncertainty of Brexit. OFCOM’s attitude has opened too - they are currently in ‘watching and waiting’ mode; a seismic shift from their previous attitude which heralded neutrality as the only priority, regardless whether it may jeopardize innovation. Although their official stance hasn’t changed, a study they’re due to publish on the revised EU Commission stance could change all of that.

Meanwhile, across the pond, the Trump administration is looking to abolish net neutrality: these days, the world’s global superpowers compete financially and America’s leaders have recognized and acted on that. If a country with the scale and resources such as the USA abolishes net neutrality, it will pave the way to utilize the new capabilities that software defined networking can bring, resulting in new business models and new ways of competing.

An ageing net neutrality policy will realize fears of being put at a competitive disadvantage for a country like the UK, which, if Brexit does go through, will only be exacerbated by having to compete against its European neighbors instead of alongside them. That’s why I expect OFCOM’s autumn statement to either declare or project a softening of its stance on net neutrality.

If both of these things happen, British service providers need to stay ahead of the curve if they want to remain competitive and attractive to suitors at the point of exit; for smaller, nimbler companies for whom SD-access is far easier to implement, the argument to do so is doubly compelling.

Whether Britain flies or fails alone on the world stage, we can be sure of one thing: turbulent, exciting times are ahead as the world of business changes fast, and forever. Businesses had better buckle up and get ready for the ride.


A religious leader and big-time fundraiser for Democratic New York City Mayor Bill de Blasio has been charged with welfare fraud for getting around $30,000 in food stamps.

Yitzchok “Isaac” Sofer, a Hasidic religious leader, hosted a fundraiser for de Blasio’s 2013 mayoral campaign at the same time he was receiving food stamps illegally.

[dcquiz] During an FBI investigation, agents found that Sofer has been on food stamps since the beginning of 2010, and received more than $30,000 in benefits from the Supplemental Nutrition Assistance Program (SNAP) since 2012, according to court documents unsealed Thursday.

On his food stamp application in 2012, Sofer claimed to make $250 a week, or about $13,000 a year, and that he had no life insurance policy. Investigators discovered, however, that Sofer did have a life insurance policy worth $1 million, and on that application he claimed to make way more than $250 dollars a week.

Sofer got the policy in 2012, however, he listed his income for 2011 at $100,000, and assets at more than $600,000, according to the criminal complaint.

Sofer still has ties with de Blasio’s office, and is listed as a government relations lobbyist for the Central United Talmudic Academy, a religious school group. The academy lobbied City Hall as recently as 2015, New York Daily News reports.

Sofer was released on $250,000 bail after being arraigned Thursday, according to the New York Post.

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How to Live with a Huge Penis by Richard Jacob

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Here’s a gift any man would be proud to receive, even if he doesn’t actually need it. (Frankly, it’s enough for someone to think he needs it.) This hilarious self-help parody is full of compassionate advice for men afflicted with Oversized Male Genitalia (OMG). Far too often, these men are banished to the fringes of society, victims of their own freakish length and girth. But Dr. Richard Jacob and Rev. Owen Thomas bring a message of tolerance and hope, along with hilarious advice on “coming out” to your family, sharing your assets with a partner, and avoiding injury in the workplace.

Complete with a daily affirmations journal and inspiring quotes from leading self-help experts, How to Live with a Huge Penis will send an uplifting message to men around the world.


The essence of self-organization is that system structure often appears without explicit pressure or involvement from outside the system. In other words, the constraints on form (i.e. organization) of interest to us are internal to the system, resulting from the interactions among the components and usually independent of the physical nature of those components. The organization can evolve in either time or space, maintain a stable form or show transient phenomena. General resource flows within self-organized systems are expected (dissipation), although not critical to the concept itself.

The field of self-organization seeks general rules about the growth and evolution of systemic structure, the forms it might take, and finally methods that predict the future organization that will result from changes made to the underlying components. The results are expected to be applicable to all other systems exhibiting similar network characteristics.

Academic Support

The Learning Change Project is a personal not for profit and without sponsors multidisciplinary initiative to support academic activities. Use the files freely for your Courses or Research. To prepare Reading Lists explore the Category List or Search for the topic of your interest. If you need any support, contact me.


#!/usr/bin/env python

"""
Copyright (c) 2006-2017 sqlmap developers (http://sqlmap.org/)
See the file 'doc/COPYING' for copying permission
"""

import re

from lib.core.enums import HTTP_HEADER
from lib.core.settings import WAF_ATTACK_VECTORS

__product__ = "EdgeCast WAF (Verizon)"

def detect(get_page):
    retval = False

    for vector in WAF_ATTACK_VECTORS:
        _, headers, code = get_page(get=vector)
        retval = code == 400 and re.search(r"\AECDF", headers.get(HTTP_HEADER.SERVER, ""), re.I) is not None
        if retval:
            break

    return retval


TTC chair Karen Stintz wasn’t always a light rail fan

City council is meeting Wednesday to vote on reviving the Sheppard LRT rather than Mayor Rob Ford’s dream of a Sheppard subway.

While TTC chair Karen Stintz has led the charge at City Hall to revive the Transit City light rail lines cancelled by Ford, she wasn’t always a fan of LRTs.

Back in 2009, Stintz told the Sun the LRT plan was “short-sighted” and argued Sheppard Ave. E., Eglinton and Scarborough-Malvern lines should be subways.

At that time, she advocated the idea subway lines be used to encourage development in areas where increased density is desirable.

“Had we taken that approach on Yonge St., we wouldn’t be the city we are today,” she said. “From a long-term city-building perspective, (Sheppard) really should be a subway, as should the Eglinton and Scarborough lines.”

“I think that we are taking a short-sighted approach to how we’re going to use this investment to benefit the city.”

Stintz of course did change her take on Transit City, even joining then-Mayor David Miller in fighting the “Save Transit City” campaign in 2010 before the municipal election.

Asked this week about her anti-LRT comments in 2009, Stintz said she had a view that LRTs were streetcars.

“I now have a better understanding of the technology and a better appreciation of how important it is to spend scarce resources wisely to improve transit across the city,” Stintz wrote in an e-mail response.

“I can also tell you that I support subways and support their construction. Our challenge is finding the resources to meet all our transit needs.”

She is a hypocrite who has gone out of her way to deceive scarborough votes…Resign Karen.. We do not want you as TTC chair….No improvement have been made during your leadership…Go back to your reality show..

Good for Stintz, educating herself to make a well informed decision rather than blindly taking someone’s word on what LRT is. Maybe everyone else who is going to post their tell tale balking of “resign!” should go do some research too.

They already have three years of funding for the Scarborough subway in the form of $1B. Surely in the next 3 years, Toronto cit ocuncil could trim a mere 2% from its operatikng budget to fund the rest over several years. We have one manager ofr every five employees in Toronto and a rearkable 50,000 staff. Why not cut 5% to built Toronto’s transit and create some 46,000 (TTC figure) person year sof work plus spinoff businesses, and jobs.

If Karen didnt know the difference what was she doing on the TTC board, just trying to snowball everyone, again and again. In 1911 a subway was first proposed, even a platform to support one built in the bloor viaduct circa 1914 implemented by the public works commissioner W Harris. ( forthought how about that) A 100 yrs of Nothing for a great city. Typical council not representing the needs of the future and Karen Stintz is just one of many on this and previous councils not pursueing whats best for the city. Maybe Karens great grachildren can hope for a subway to pass by. Oh wait another lifetime for a LRT.

Yeah, that’s what people do when they get information that is contradictory to what they believe is true. They get more information and then decide what they believe. It’s called thinking.
It doesn’t mean that you are right necessarily, but the odds are in your favour.

@Andy …surely Sheppard would have to support the need for an actual subway before building it? Which let’s face it the stubway was just put in because Lastman has a big mouth.

Surely everyone in the city should just subsidize a transit line that _will never break even_ Surely! How about no? How about find a funding model to build a DRL that makes sense instead? How about building transit that fits the area it serves?

In reality, the subway could have been done and completed by now, all the funds lost when Smitherman had the Health Portfolio on Provincial level. Now we appear to see a similiar “POWER EGO TRIP” with Ms Stintz at the helm. Does Ms. Stintz not realize this amount of money is for “long term investment”? Subways are like email compared to sending letters by mail called snail mail.
But apparently some councillors still think in the snail mail mode. Wake up were in 2012!!!

JUST CHECK OUT CITY OF TORONTO’S WEBSITE ON COLLE AND STINTZ……you wonder if these two
are self serving?

Leave a comment

Don Peat

Don Peat is the City Hall bureau chief for the Toronto Sun. He covers municipal affairs at Toronto City Hall, a beat that has him writing about everything from garbage to transit to taxes to multimillion-dollar spending scandals.


Q:

asynchronous http request handling with tomcat and spring

It's my first SO question so be patient with me :)
I'm trying to create a service that:

Receives HTTP GET requests containing a URL to query
For a single GET request the service extracts the URL
Queries a local DB about the URL
If a result was found in the DB it will return it to the client and if not it will need to query some external services (that may take relatively long time to respond)
Return the result of the URL to the client

I'm running this on a virtual machine and Tomcat7 with spring.
I'll apologize in advance and mention that I'm pretty new to Tomcat
Anyway, I'm expecting a lot of concurrent GET requests to this service (hundreds of thousands of simultaneous requests)
What I'm basically trying to achieve is to make this service as scalable as possible (and if that's not possible then at least a service that can handle hundreds of thousands of simultaneous requests)
I've been reading A LOT about asynchronous requests handling in services and especially in Tomcat but I have some things that are still unclear to me:

From the official tomcat website it seems that Tomcat contains number of acceptor threads and number of working threads.
If so, why should I use AsyncContext? Whats the benefit of releasing a Tomcat's working thread and occupying a different thread in my application to do the exact same actions? (there's still 1 active thread in the system)
Somewhat similar to the first question but are there any benefits for creating the AsyncContext and using it with a different thread? (a thread from a thread pool created in my application)
Regarding the same issue, I've seen here that I can also return a Callable or a DeferredResult and process it with either one of Tomcat's threads or with one of my own threads. Are there any benefits for returning a Callable or using a DeferredResult over just processing the AsyncContext from the requests?
Also, If I decide to return a callable, from what thread pool does Tomcat gets the thread to process my callable? Are the threads being used here the same working threads from Tomcat that I previously mentioned? If so, what benefits do I get from releasing one Tomcat working thread and using a different one instead?
I've seen from Oracle's documentation that I can pass AsyncContext a Runnable object that will be processed concurrently, From where do the threads used to execute this Runnable come from? Do I have any control over it? Also, any benefits to passing the AsyncContext a Runnable over just passing the AsyncContext to one my threads?

I apologize for asking so many questions regarding the same things but me and my colleagues are arguing over these things for over a week without any concrete answer.
I have 1 more general question:
What do you think is the best way to make the service I described scalable? (putting aside adding more machines at the moment), could you post any examples or references for the purposed solution?
I'd post more links of links I've been looking at but my current reputation doesn't allow it.
I'll be grateful for any understandable references or for concrete examples and I'll obviously be happy to clarify on any relevant issue
Cheers!

A:

There are a lot of questions packed into this, but I'll try to address some of them.
Asynchronous I/O is a good thing, especially on servers that serve large volumes of requests - it allows you to use fewer threads to process more requests.  In the case of a proxy such as you are writing, you really want your HTTP client (that makes the requests to foreign URLs) to be asynchronous as well, so that neither processing the request nor receiving the remote response involves blocking I/O.
That said, you may have a harder time doing this stuff with Tomcat or Java EE servers in general, which have had asynchronous I/O bolted onto them as an afterthought, than using a framework like Netty that is asynchronous from the ground up.  As the author of a framework which builds on top of Netty, I'm a bit biased.
To demonstrate how little code you'd need to do what you describe, I wrote a small server that does what you describe here in 3 Java source files and put it on github - it builds a standalone JAR you can run with java -jar to try it out, and I tried to comment it clearly.
What it comes down to is, networked applications spend most of their time waiting for I/O to happen.  In the case of a proxy in particular, with traditional, threaded I/O, you would get a request, and the thread that received the request would be responsible for answering it synchronously - that means, if it has to make a network request to another server, that thread is blocked waiting for the answer to come from the remote server.  Meaning that thread can't be used for anything else.  So, if you have 10 threads, and all of them are waiting on responses, your server can't answer any more requests until one of them finishes and frees up a thread.  With asynchronous I/O, you get a callback when some I/O completes.  In other words, instead of standing still until the OS flushes your data to the socket and out the network card, your code simply gets a friendly tap on the shoulder when there is something to do (like a response arriving from your proxy request).  While your code is waiting for that HTTP request to complete, the thread that sent the proxy request is free to be used to handle another request  That means one thread can do a little work on one request, do a little work on another, and another, and eventually finish the first request.  Since threads are a finite resource provided by your operating system, this allows you to do a lot more with a lot less hardware.
As to Callable vs. DeferredResult, using a Callable just moves when the work happens around (the Callable gets executed later, on some thread or other, but is still expected to do return a result synchronously);  DeferredResult sounds more like what you'd need, since that allows your code to go off and do whatever work it wants, and then set the result (triggering completion of the response) whenever it has something to set.
Honestly, I think if you want to implement this really efficiently, you'd be better off staying away from the Java EE stack - so much of it has baked in assumptions that I/O is synchronous that trying to do async stuff with it is swimming upstream (for example, JDBC has synchronous I/O baked into its bones - if you really want this to scale and you want to use an SQL database, you'd be better off with something like this ).
For another example of using Netty for this sort of thing, see the tiny-maven-proxy project - the code is less pretty, but it shows an example of doing an HTTP proxy where the response body is fed to the client chunk-by-chunk, as it arrives - so you never actually pull the full response body into memory, meaning even requests with huge responses won't run the proxy out of memory.  Tiny-maven-proxy also caches on the filesystem.  I didn't do those things in the demo because it would have made the code more complicated.


Griqualand-East Commando

Griqualand East Commando was a light infantry regiment of the South African Army. It formed part of the South African Army Infantry Formation as well as the South African Territorial Reserve.

History

Origins

Rifle Association
Griqualand East Commando can trace its origin to a Defence Rifle Association formed by a Captain Woods of the Cape Mounted Rifles around 1884. Its primary aim was for the farming community to be able to defend themselves against hostile tribes that stole their cattle.

Operations

With the UDF
By 1948, the Griqualand East Rifle Association was formed to manage local area defence. In 1953, Mount Currie Rifle Association in Kokstad amalgamated with the Grqiualand East Rifle Association which saw the formation of the Commando in Kokstad.

With the SADF
By 1984 however the commando moved to Cedarville as a disused school had become available for accommodation.

Area of responsibility
Griqualand East Commando was responsible for the magisterial district of Mount Currie.

Higher headquarters
The commando was under the command of Natal Command from 1930 to 1950 but then placed under Eastern Province Command, this situation reverted again in 1960 due to the establishment of the Transkei.

Freedom of entry
The Freedom of the town of Kokstad was granted to the commando in 1993.

With the SANDF

Disbandment
This unit, along with all other Commando units was disbanded after a decision by South African President Thabo Mbeki to disband all Commando Units. The Commando system was phased out between 2003 and 2008 "because of the role it played in the apartheid era", according to the Minister of Safety and Security Charles Nqakula.

Unit Insignia

Leadership

 Cmdt A.L.A. Maartins 1952-1972
 Cmdt J.H. Venter 1973-1977
 Cmdt S.A. Ponder 1977-1981
 Lt Col D.W. Schoeman 1982-

References

See also
 South African Commando System

Category:Infantry regiments of South Africa
Category:South African Commando Units