different sector \[($b$,$c$), ($\beta^\mp$,$\gamma^\pm$), and ($\eta$,$\xi$) respectively\] are separately indicated. We can see that the ghost number anomaly vanishes due to a cancellation of the background charges. Our formulation reproduces the desired answer as is expected.

Let us now turn to the anomaly associated with the conservation of the BRST supercurrent. We define the BRST supercurrent as \[\] $$\eqalign{
  j_B(Z)&\equiv C\left(T^X+{1\over2}T^{\rm gh}\right)
  +{1\over4}\Diminus\left[C\left(\Diplus C\right)B\right]
  +{1\over4}\Diplus\left[C\left(\Diminus C\right)B\right]
\cr
  &\equiv J_B(Z)+\widehat\jmath_B(Z).
\cr
}
\eqn\twosixteen$$ To see the structure of the BRST anomaly, we call the first term in the first line in  as $J_B(Z)$ and the total divergence parts as $\widehat\jmath_B(Z)$. We should note here that we chose the total divergence parts $\widehat\jmath_B(B)$ (which do not affect to the BRST charge $Q_B$) by $$j_B(Z)=-\left\{Q_B,j_{\rm gh}(Z)\right\},
\eqn\twoseventeen$$ to make the BRST current manifestly BRST invariant if $Q_B^2=0$. In this sense the above choice is the most symmetric one and this choice of $\widehat\jmath_B(Z)$ is crucial for our conclusion.

We also define the components of the BRST supercurrent as $$\eqalign{
  &J_B(Z)\equiv J_B^0(z)+\thetaminus J_B^++\thetaplus J_B^-(z)
  +\thetaminus\thetaplus J_B^{+-}(z),
\cr
  &\widehat\jmath_B(Z)\equiv\widehat\jmath_B^0(z)+\thetaminus\widehat
\jmath_B^+
  +\thetaplus\widehat\jmath_B^-(z)
  +\thetaminus\thetaplus\widehat\jmath_B^{+-}(z).
\cr
}
\ee$$ The explicit form of the component currents of $J_B(Z)$ becomes: $$\eqalign{
  &J_B^0(z)={1\over2}c\left[\psiminusmu\psiplusmu
   -i\partial(c\eta)+{1\over2}\gammaplus\betaminus
   -{1\over2}\gammaminus\betaplus\right],
\cr
  &J_B^+(z)=-{1\over2}c\biggl[-i\partial\Ymu\psiplusmu
   +\partial\Xmu\psiplusmu-\partial\left(\gammaplus\eta\right)
   +i\partial\left(c\betaplus\right)-{1\over2}i\gammaplus b
   +{1\over2}\gammaplus\partial\eta
