Why is the determinant not integrated over in Faddeev-Popov? In Peskin & Schroeder chapter 16.2 the authors go through the computation of the non-Abelian gauge boson propagator using the Faddeev-Popov procedure as is done for the QED case. The difference here, is that our functional determinant is not just a constant which we can cancel out. It turns out that this functional determinant gives an extra contribution to the Feynman rules of the theory. My question here is the following:
During the derivation we arrive at
$$
\begin{aligned}\int{\mathcal{D}Ae^{iS[A]}}&=\int\mathcal{D}Ae^{iS[A]}\int{\mathcal{D}\alpha(x)\delta(G(A^\alpha))\det\left(\frac{\delta G(A^\alpha)}{\delta\alpha}\right)}\\
&=\int\mathcal{D}\alpha(x)\int{\mathcal{D}Ae^{iS[A]}}\delta(G(A^\alpha))\det\left(\frac{\delta G(A^\alpha)}{\delta\alpha}\right).
\end{aligned}
$$
Now from here we use the fact that $\mathcal{D}A^\alpha=\mathcal{D}A$ and $S[A^\alpha]=S[A]$ where $A^\alpha$ is the gauge transform of $A$. And now we can rewrite the functional integral as
$$
\left(\int{\mathcal{D}\alpha}\right)\int{\mathcal{D}A^\alpha e^{iS[A^\alpha]}}\delta(G(A^\alpha))\det\left(\frac{\delta G(A^\alpha)}{\delta\alpha}\right)=\left(\int{\mathcal{D}\alpha}\right)\int{\mathcal{D}A e^{iS[A]}}\delta(G(A))\det\left(\frac{\delta G(A^\alpha)}{\delta\alpha}\right)
$$
where we just relabel the integration variable $A^\alpha$ to $A$. What about the part where we multiply with the determinant? Since that depends on $A^a_\mu$ shouldn't we relabel that? But if we do that then the derivation doesn't work because we need the gauge transformed determinant.
Would this be the case because initially, the determinant was in the integral of $\int{\mathcal{D}\alpha}$ instead of the integral of $\int{\mathcal{D}A\;e^{iS[A]}}$?
 A: In the Lagrangian formalism of path integral quantization, one invokes the formula $$\int d\theta\,\delta(f(\theta))=\int df\det\Bigg|\frac{d\theta}{df}\Bigg|\delta(f(\theta))=\det\Bigg|\frac{d\theta}{df}\Bigg|_{f=0}. \tag{$\ast$}$$
Now consider the naive partition function $$\mathcal{Z}=\int\mathcal{D}[A]e^{-S[A]}. \tag{1}$$
The action $S[A]$ and the functional integral measure $\mathcal{D}[A]$ must be gauge invariant under an arbitrary gauge transformation $$A[U]=U^{-1}dU+U^{-1}AU\quad\mathrm{or}\quad\delta_{U}A=d\,\delta U+[A,\delta U], \tag{$\star$}$$
and $\mathcal{D}[A]\equiv\prod_{\mu,a,x}dA^{a}_{\mu}(x)$.
Next, consider a "haar measure" on the (infinite dimensional) Lie group of gauge transformations ($\star$), i.e $$\mathcal{D}[U]=\mathcal{D}[UU^{\prime}];\quad\mathrm{and}\quad\mathcal{D}[U]\equiv\prod_{x}dU(x),$$
and define the Faddeev-Popov determinant via the following functional integral identity $$1=\Delta[A]\int\mathcal{D}[U]\,\delta[\mathcal{F}(A[U])], \tag{2}$$
where $\mathcal{F}(A[U])$ is known as the gauge fixing condition to be specified.

Claim: The Faddeev-Popov determinant $\Delta[A]$ is gauge invariant. 
proof: It can be shown as follows $$\Delta[A]^{-1}=\int\mathcal{D}[U]\,\delta[\mathcal{F}(A[U])],\quad\mathrm{hence}\quad\Delta[A[U]]^{-1}=\int\mathcal{D}[U^{\prime}]\,\delta[\mathcal{F}(A[UU^{\prime}])].$$
But since $\mathcal{D}U$ is gauge invariant, one has $$\Delta[A[U]]^{-1}=\int\mathcal{D}[UU^{\prime}]\,\delta[\mathcal{F}(A[UU^{\prime}])]=\Delta[A]^{-1}.$$

Now insert the functional integral identity (2) into the partition function (1), one has
\begin{align}
\mathcal{Z}&=\int\mathcal{D}[A]e^{-S[A]} \\
&=\int\mathcal{D}[A]\Delta[A]\int\mathcal{D}[U]\,\delta[\mathcal{F}(A[U])]e^{-S[A]} \\
&=\int\mathcal{D}[U]\int\mathcal{D}[A]\left(\Delta[A]\delta[\mathcal{F}(A[U])]e^{-S[A]}\right). 
\end{align}

Now observe that the integrand $$\int\mathcal{D}[A]\left(\Delta[A]\delta[\mathcal{F}(A[U])]e^{-S[A]}\right)$$
under the integral $\int\mathcal{D}[U]$ is actually independent of $U$, therefore it can be replaced by $$\int\mathcal{D}[A[U]]\left(\Delta[A[U]]\delta[\mathcal{F}(A[U])]e^{-S[A[U]]}\right)=\int\mathcal{D}[A]\left(\Delta[A]\delta[\mathcal{F}(A)]e^{-S[A]}\right).$$

Thus, the partition function can be written as $$\mathcal{Z}=\int\mathcal{D}[U]\int\mathcal{D}[A]\left(\Delta[A]\delta[\mathcal{F}(A)]e^{-S[A]}\right). \tag{3}$$
Next, use the functional version of the formula ($\ast$), one has
\begin{align}
\Delta[A]^{-1}&=\int\mathcal{D}[\mathcal{F}]\mathrm{Det}\Bigg|\frac{\delta U}{\delta\mathcal{F}(A[U])}\Bigg|\delta[\mathcal{F}] \\
&=\int\mathcal{D}[\mathcal{F}]\mathrm{Det}\Bigg|\frac{\delta\mathcal{F}(A[U])}{\delta U}\Bigg|^{-1}\delta[\mathcal{F}] \\
&=\mathrm{Det}\Bigg|\frac{\delta\mathcal{F}(A[U])}{\delta U}\Bigg|^{-1}\Bigg|_{\mathcal{F}(A[U])=0},
\end{align}
i.e $$\Delta[A]=\mathrm{Det}\Bigg|\frac{\delta\mathcal{F}(A[U])}{\delta U}\Bigg|_{\mathcal{F}(A[U])=0}.$$
One can pick a gauge fixing condition $\mathcal{F}(A[U])$ such that $\mathcal{F}(A[U])=0$ at $U=\mathrm{id}$.
Since from the above expression one finds that only infinitesimal gauge transformations are relevant in calculation, one can safely assume $$U(x)=\exp\left\{i\sum_{a}T^{a}\Lambda_{a}(x)\right\}, \tag{4}$$
where $\left\{T_{a}\right\}_{a=1,\cdots,N}$ is a basis of the Lie algebra of the gauge group. Then, the Fadeev-Popov determinant can be chosen such that $$\Delta[A]=\mathrm{Det}\Bigg|\frac{\delta\mathcal{F}(A[U])}{\delta U}\Bigg|_{U=\mathrm{id}}$$
Then, using the functional chain-rule and linearity of determinant, one has
$$\frac{\delta\mathcal{F}(A[U](x))}{\delta U(y)}\Bigg|_{U=\mathrm{id}}=\sum_{a}\int d^{4}z\frac{\delta\mathcal{F}(A[U](x))}{\delta\Lambda_{a}(z)}\Bigg|_{\Lambda=0}\frac{\delta\Lambda_{a}(z)}{\delta U(y)}\Bigg|_{\Lambda=0}.$$
Notice that the factor on the right is the inverse of $$\left(\frac{\delta U(y)}{\delta\Lambda_{a}(z)}\right)\Bigg|_{\Lambda=0}=iT^{a}\delta(y-z),$$
which is a Lie algebra-valued constant. The above equation is an (infinite-dimensional) linear transformation on $$\mathcal{M}\equiv\frac{\delta\mathcal{F}(A[U])}{\delta\Lambda}.$$
Thus, up to some infinite constant, one can replace $\Delta[A]$ by $\mathrm{Det}\mathcal{M}$ in the partition function.
More precisely, one has $$\Delta[A]=\mathrm{Det}\Bigg|\frac{\delta\mathcal{F}(A[U])}{\delta U}\Bigg|_{U=\mathrm{id}}=\mathrm{Det}(\mathcal{M}\cdot^{-1})=\mathrm{Det}\mathcal{M},$$
where
\begin{align}
(\mathcal{M}\cdot^{-1})(x,y)&=\int d^{4}z\frac{\delta\mathcal{F}(A[U](x))}{\delta\Lambda(z)}\Bigg|_{\Lambda=0}\cdot\frac{\delta\Lambda(z)}{\delta U(y)}\Bigg|_{\Lambda=0} \\
&=\int d^{4}z\mathcal{M}(x,z)^{-1}(z,y).
\end{align}
Using the functional chain-rule, one obtains
\begin{align}
\mathcal{M}^{ab}(x,y)&\equiv\int d^{4}z\left(\frac{\delta\mathcal{F}^{a}(A[U](x))}{\delta A[U]^{c}_{\mu}(z)}\frac{\delta A[U]^{c}_{\mu}(z)}{\delta\Lambda_{b}(y)}\right)\Bigg|_{\Lambda=0} \\
&=\int d^{4}z\frac{\delta\mathcal{F}^{a}(A(x))}{\delta A^{c}_{\mu}(z)}\left(\frac{\partial}{\partial z_{\mu}}\delta^{cb}+\sum_{d}f^{cbd}A_{d\mu}(z)\right)\delta(z-y). \tag{5}
\end{align}
Also notice that under the change of variables, $$\mathcal{D}[U]=\mathrm{Det}\left(\frac{\delta U}{\delta\Lambda}\right)\mathcal{D}[\Lambda],$$
the Jacobian factor is an infinite constant (independent of gauge fields $A_{\mu}^{a}(x)$), which can be omitted in the functional integral.
Plugging (5) back into (3), one has $$\mathcal{Z}=\int\mathcal{D}[\Lambda]\int\mathcal{D}[A]\left(\mathrm{Det}\mathcal{M}\cdot\delta[\mathcal{F}(A)]\cdot e^{-S[A]}\right).$$
But the integrand $$\int\mathcal{D}[A]\left(\mathrm{Det}\mathcal{M}\cdot\delta[\mathcal{F}(A)]\cdot e^{-S[A]}\right)$$
under the integral $\int\mathcal{D}[\Lambda]$ is independent of $\Lambda$, thus the integral $\int\mathcal{D}[\Lambda]$ of gauge orbits only produces an infinite constant factor, which can be omitted.
Finally, one obtains the gauge-fixed partition function $$\mathcal{Z}=\int\mathcal{D}[A]\left(\mathrm{Det}\mathcal{M}\cdot\delta[\mathcal{F}(A)]\cdot e^{-S[A]}\right).$$
In your case, one can pick up the Lorenz gauge $$\mathcal{F}(A)=\partial_{\mu}A^{\mu}=0$$
in QED, and the Faddeev-Popov matrix is $$\mathcal{M}(x,y)=\Box\,\delta(x-y)$$
which is a constant.
More generally, in the non-Abelian case, since the $A^{a}_{\mu}(z)$ appears in the Faddeev-Popov determinant, the determinant cannot be factored out in the functional integral, and produces non-trivial interactions between photons and ghost fermions.
The gauge fixing procedure is even clearer in the canonical approach of the path-integral. TO BE CONTINUED
A: As in the Abelian case, the path integral becomes
\begin{align}
\int \mathcal{D} A \; \int \mathcal{D}\alpha \; \delta [ G(A^\alpha)]  \det \left( \frac{\delta  G(A^\alpha)}{\delta \alpha} \right) \exp\left[ i \int d^4x\; \left( -\frac{1}{4} \big( F(A)_{\mu\nu}^a\big)^2\right)\right]
\end{align}
and we can  change the order of integration $A' = A^\alpha$:
\begin{align}
\int \mathcal{D}\alpha \; \int \mathcal{D} A \; \delta [ G(A')]  \det \left( \frac{\delta  G(A')}{\delta \alpha} \right) \exp\left[ i \int d^4x\; \left( -\frac{1}{4} \big( F(A)_{\mu\nu}^a\big)^2\right)\right]
\end{align}
Contrary to the Abelian  case the determinant is not independent of the gauge fields and we cannot take it outside of the gauge field integration. As in QED we use the fact that the Lagrangian is invariant under gauge transformations and we can just replace $F(A)$ by $F(A')$ in the action. In QED we can also change the measure $\mathcal{D}A$ by $\mathcal{D}A'$ as the change in integration variables was just linear shift.  In this case the change in integration variables is a bit more complicated and given by
\begin{align}
\big( A^\alpha \big) ^a_{\mu} = A_\mu^a +\frac{1}{g} \partial_\mu \alpha^a + f^{abc} A^b_\mu\alpha^c =  A_\mu^a + \frac{1}{g}D_\mu\alpha^a 
\end{align}
It consist of a linear shift followed by a rotation in internal space. Both these operations preserve the measure and so we have $\mathcal{D}A=\mathcal{D}A'$ as well. We can thus write the path integral as
\begin{align}
\int \mathcal{D}\alpha \; \int \mathcal{D} A' \; \delta [ G(A')]  \det \left( \frac{\delta  G(A')}{\delta \alpha} \right) \exp\left[ i \int d^4x\; \left( -\frac{1}{4} \big( F(A')_{\mu\nu}^a\big)^2\right)\right]
\end{align}
and can now simply replace the integration variable $A'$ by $A$ to obtain
\begin{align}
\int \mathcal{D}\alpha \; \int \mathcal{D} A \; \delta [ G(A)]  \det \left( \frac{\delta  G(A)}{\delta \alpha} \right) \exp\left[ i \int d^4x\; \left( -\frac{1}{4} \big( F(A)_{\mu\nu}^a\big)^2\right)\right]
\end{align}
In the Abelian case, the determinant is independent of the gauge field $A$ and can be taken out of the gauge field integration. It contributes to an overall normalisation constant and we can simply ignore it, as it is factored out in correlation functions and scattering amplitudes. In the non-Abelian case we cannot just ignore this determinant as it depends on the gauge field. We have
\begin{align}
\frac{\delta G (A^\alpha)}{\delta \alpha} &= \frac{\delta }{\delta \alpha} \left[ \partial^\mu \big( A^\alpha \big)^a_\mu(x) - \omega^a(x) \right] \nonumber\\
&= \partial^\mu \frac{\delta }{\delta \alpha}  \big( A^\alpha \big)^a_\mu(x) =\partial^\mu \frac{\delta }{\delta \alpha} \big[ A^a_\mu + \frac{1}{g} D_\mu \alpha \big]= \frac{1}{g}\partial^\mu D_\mu
\end{align}
In the Abelian case the covariant derivative equals the ordinary derivative and we recover, of course, the QED result.
We chose to rewrite this determinant as a functional integral over anti-commuting fields $c$ and $\bar{c}$.
\begin{equation}
{
\det \left( \frac{1}{g} \partial^\mu D_\mu \right) = \int \mathcal{D} c\, \mathcal{D}\bar{c}\, e^{i\int d^4x\, \bar{c}\big( - \partial^\mu D_\mu \big) c} } \label{eq:ymhhgwpfdg}
\end{equation}
