in the strong disordered case, but with a field-dependent smaller exponent \[18\]. To show this, let us briefly explain how to evaluate the conductivity near a VG transition. As accepted even through the studies \[6\] at higher temperatures, the conductivity $\sigma_{ij}$ may be separated into the quasiparticle part $\sigma_{n, \, ij}$ and the superconducting fluctuation part $\sigma_{s, \, ij}$, and, deep in the liquid regime of clean systems, $\sigma_{s, \, ij}$ can be expressed as a sum of the pinning-free contribution $\sigma_{F, ij}$ and the glass fluctuation part $\sigma_{G, ij}$ so that $\sigma_{ij} \simeq \sigma_{n, \, ij} +
\sigma_{F, ij} + \sigma_{G, ij}$ \[17\]. The dynamics of $\psi$-field is incorporated according to the TDGL equatioin, or equivalently the quantum TDGL action \[17,36\] $${{S_{\rm QLD}} \over \hbar}=d \sum_j \int d^2r \beta \sum_\omega
(\gamma_1 |\omega| + {\rm i} \gamma_2 \omega ) |\psi_j({\bf r},
\omega)|^2 +
\int_0^{\hbar \beta} {{d\tau} \over \hbar} \biggl[ {\cal H}_{\rm
LD}(\psi \to \psi(\tau))$$ $$+ {\cal H}_{rp}(\psi \to \psi(\tau)) \, \biggr], \eqno(2.18)$$ for the LD model, where $\beta=1/(k_{\rm B} T)$, $\gamma_1 > 0$, and $\omega$ denotes Matsubara frequency. As first found in Ref.37, the vortex flow conductivities $$\sigma_{F, xx}=R_q^{-1} {{\gamma_1 \, \phi_0} \over {b \, B}} (-
\mu_0) \eqno(2.19)$$ and 