{f_j({\bf r}) f_l({\bf r}')}}=d^{-1}
\Delta_\Phi^{(p)} \delta^{(2)}({\bf r} - {\bf r}')
\, \delta_{j, l}$. Roughly speaking, $\chi_G$ in 3D case is given by replacing $\Delta/\mu^2$ in eq.(2.13) by $\Delta^{(p)}/\mu^{3/2}$ when, for simplicity, neglecting a $\Delta_\Phi$ term. If, as in 2D case, $N_{\rm cor}$ is identified with the dimensionless positional correlation area perpendicular to ${\bf B}$ found in the collective pinning theory (in type II limit) \[33\], we obtain $$I_{\rm irr} \simeq \Delta_{\rm eff} (\beta_A - 1) \exp(c_1 \,
\Delta_{\rm eff}^{-1}) \eqno(2.15)$$ along the first order line expected in LLL (see eq.(2.17) below), where $c_1$ is a positive constant. Since eq.(2.15) is divergent in $\Delta_{\rm eff} \to 0$ limit, it implies that the glass transition due to point disorder, the so-called vortex-glass (VG) transition, will occur more suddenly in cleaner systems with smaller $\Delta_{\rm eff}$ and that the first order transition in clean limit should be a glass transition simultaneously. Further, the exponential $\Delta_{\rm eff}$-dependence of $N_{\rm cor}$ suggests that this pinning dependence is stronger than the prefactor $\Delta_{\rm eff}$ in eq.(2.15). Since $N_{\rm cor}$ will decrease down to a constant of order unity with increasing $\Delta_{\rm
eff}$, and $\beta_A$ depends only weakly on $\Delta_{\rm eff}$, it is expected that $I_{\rm irr}$ 