Polyakov action

Template:Short description Template:String theory In physics, the Polyakov action is an action of the two-dimensional conformal field theory describing the worldsheet of a string in string theory. It was introduced by Stanley Deser and Bruno Zumino and independently by L. Brink, P. Di Vecchia and P. S. Howe in 1976,<ref>Template:Cite journal</ref><ref>Template:Cite journal</ref> and has become associated with Alexander Polyakov after he made use of it in quantizing the string in 1981.<ref>Template:Cite journal</ref> The action reads:

<math>\mathcal{S} = \frac{T}{2} \int\mathrm{d}^2\sigma\, \sqrt{-h}\,h^{ab} g_{\mu\nu}(X) \partial_a X^\mu(\sigma) \partial_b X^\nu(\sigma),</math>

where <math>T</math> is the string tension, <math>g_{\mu\nu}</math> is the metric of the target manifold, <math>h_{ab}</math> is the worldsheet metric, <math>h^{ab}</math> its inverse, and <math>h</math> is the determinant of <math>h_{ab}</math>. The metric signature is chosen such that timelike directions are + and the spacelike directions are −. The spacelike worldsheet coordinate is called <math>\sigma</math>, whereas the timelike worldsheet coordinate is called <math>\tau</math>. This is also known as the nonlinear sigma model.<ref name="Frie80">Template:Cite journal</ref>

The Polyakov action must be supplemented by the Liouville action to describe string fluctuations.

Global symmetriesEdit

N.B.: Here, a symmetry is said to be local or global from the two dimensional theory (on the worldsheet) point of view. For example, Lorentz transformations, that are local symmetries of the space-time, are global symmetries of the theory on the worldsheet.

The action is invariant under spacetime translations and infinitesimal Lorentz transformations Template:Ordered list where <math> \omega_{\mu \nu} = -\omega_{\nu \mu} </math>, and <math> b^\alpha </math> is a constant. This forms the Poincaré symmetry of the target manifold.

The invariance under (i) follows since the action <math> \mathcal{S} </math> depends only on the first derivative of <math> X^\alpha </math>. The proof of the invariance under (ii) is as follows:

<math>\begin{align}

 \mathcal{S}'
   &= {T \over 2}\int \mathrm{d}^2\sigma\, \sqrt{-h}\, h^{ab} g_{\mu \nu} \partial_a \left( X^\mu + \omega^\mu_{\ \delta} X^\delta \right) \partial_b \left( X^\nu + \omega^\nu_{\ \delta} X^\delta \right) \\
   &= \mathcal{S} + {T \over 2}\int \mathrm{d}^2\sigma\, \sqrt{-h}\, h^{ab} \left( \omega_{\mu \delta} \partial_a X^\mu \partial_b X^\delta + \omega_{\nu \delta} \partial_a X^\delta \partial_b X^\nu \right) + \operatorname{O}\left(\omega^2\right) \\
   &= \mathcal{S} + {T \over 2}\int \mathrm{d}^2\sigma\, \sqrt{-h}\, h^{ab} \left( \omega_{\mu \delta} + \omega_{\delta \mu } \right) \partial_a X^\mu \partial_b X^\delta + \operatorname{O}\left(\omega^2\right) \\
   &= \mathcal{S} + \operatorname{O}\left(\omega^2\right).

\end{align}</math>

Local symmetriesEdit

The action is invariant under worldsheet diffeomorphisms (or coordinates transformations) and Weyl transformations.

DiffeomorphismsEdit

Assume the following transformation:

<math> \sigma^\alpha \rightarrow \tilde{\sigma}^\alpha\left(\sigma,\tau \right). </math>

It transforms the metric tensor in the following way:

<math> h^{ab}(\sigma) \rightarrow \tilde{h}^{ab} = h^{cd} (\tilde{\sigma})\frac{\partial {\sigma}^a}{\partial \tilde{\sigma}^c} \frac{\partial {\sigma}^b}{\partial \tilde{\sigma}^d}. </math>

One can see that:

<math>

 \tilde{h}^{ab} \frac{\partial}{\partial {\sigma}^a} X^\mu(\tilde{\sigma}) \frac{\partial}{\partial \sigma^b} X^\nu(\tilde{\sigma}) =
 h^{cd} \left(\tilde{\sigma}\right)\frac{\partial \sigma^a}{\partial \tilde{\sigma}^c} \frac{\partial \sigma^b}{\partial \tilde{\sigma}^d} \frac{\partial}{\partial \sigma^a} X^\mu(\tilde{\sigma})\frac{\partial}{\partial {\sigma}^b} X^\nu(\tilde{\sigma}) =
 h^{ab}\left(\tilde{\sigma}\right)\frac{\partial}{\partial \tilde{\sigma}^a}X^\mu(\tilde{\sigma}) \frac{\partial}{\partial \tilde{\sigma}^b} X^\nu(\tilde{\sigma}).

</math>

One knows that the Jacobian of this transformation is given by

<math> \mathrm{J} = \operatorname{det} \left( \frac{\partial \tilde{\sigma}^\alpha}{\partial \sigma^\beta} \right), </math>

which leads to

<math>\begin{align}

 \mathrm{d}^2 \tilde{\sigma} &= \mathrm{J} \mathrm{d}^2 \sigma \\
                           h &= \operatorname{det} \left( h_{ab} \right) \\
       \Rightarrow \tilde{h} &= \mathrm{J}^2 h,

\end{align}</math> and one sees that

<math> \sqrt{-\tilde{h}} \mathrm{d}^2 {\sigma} = \sqrt{-h \left(\tilde{\sigma}\right)} \mathrm{d}^2 \tilde{\sigma}. </math>

Summing up this transformation and relabeling <math> \tilde{\sigma} = \sigma </math>, we see that the action is invariant.

Weyl transformationEdit

Assume the Weyl transformation:

<math> h_{ab} \to \tilde{h}_{ab} = \Lambda(\sigma) h_{ab}, </math>

then

<math>\begin{align}

                                   \tilde{h}^{ab} &= \Lambda^{-1}(\sigma) h^{ab}, \\
 \operatorname{det} \left( \tilde{h}_{ab} \right) &= \Lambda^2(\sigma) \operatorname{det} (h_{ab}).

\end{align}</math> And finally:

<math> \mathcal{S}', </math>	<math> = {T \over 2}\int \mathrm{d}^2 \sigma \sqrt{-\tilde{h}} \tilde{h}^{ab} g_{\mu\nu} (X) \partial_a X^\mu (\sigma) \partial_b X^\nu(\sigma), </math>
	<math> = {T \over 2}\int \mathrm{d}^2 \sigma \sqrt{-h} \left( \Lambda \Lambda^{-1} \right) h^{ab} g_{\mu \nu} (X) \partial_a X^\mu (\sigma) \partial_b X^\nu(\sigma) = \mathcal{S}. </math>

And one can see that the action is invariant under Weyl transformation. If we consider n-dimensional (spatially) extended objects whose action is proportional to their worldsheet area/hyperarea, unless n = 1, the corresponding Polyakov action would contain another term breaking Weyl symmetry.

One can define the stress–energy tensor:

<math> T^{ab} = \frac{-2}{\sqrt{-h}} \frac{\delta S}{\delta h_{ab}}. </math>

Let's define:

<math> \hat{h}_{ab} = \exp\left(\phi(\sigma)\right) h_{ab}. </math>

Because of Weyl symmetry, the action does not depend on <math> \phi </math>:

<math> \frac{\delta S}{\delta \phi} = \frac{\delta S}{\delta \hat{h}_{ab}} \frac{\delta \hat{h}_{ab}}{\delta \phi} = -\frac12 \sqrt{-h} \,T_{ab}\, e^{\phi}\, h^{ab} = -\frac12 \sqrt{-h} \,T^a_{\ a} \,e^{\phi} = 0 \Rightarrow T^{a}_{\ a} = 0, </math>

where we've used the functional derivative chain rule.

Relation with Nambu–Goto actionEdit

Writing the Euler–Lagrange equation for the metric tensor <math> h^{ab} </math> one obtains that

<math> \frac{\delta S}{\delta h^{ab}} = T_{ab} = 0. </math>

Knowing also that:

<math> \delta \sqrt{-h} = -\frac12 \sqrt{-h} h_{ab} \delta h^{ab}. </math>

One can write the variational derivative of the action:

<math> \frac{\delta S}{\delta h^{ab}} = \frac{T}{2} \sqrt{-h} \left( G_{ab} - \frac12 h_{ab} h^{cd} G_{cd} \right), </math>

where <math> G_{ab} = g_{\mu \nu} \partial_a X^\mu \partial_b X^\nu </math>, which leads to

<math>\begin{align}

 T_{ab} &= T \left( G_{ab} - \frac12 h_{ab} h^{cd} G_{cd} \right) = 0, \\
 G_{ab} &= \frac12 h_{ab} h^{cd} G_{cd}, \\
      G &= \operatorname{det} \left( G_{ab} \right) = \frac14 h \left( h^{cd} G_{cd} \right)^2.

\end{align}</math>

If the auxiliary worldsheet metric tensor <math>\sqrt{-h}</math> is calculated from the equations of motion:

and substituted back to the action, it becomes the Nambu–Goto action:

<math> S = {T \over 2}\int \mathrm{d}^2 \sigma \sqrt{-h} h^{ab} G_{ab} = {T \over 2}\int \mathrm{d}^2 \sigma \frac{2 \sqrt{-G}}{h^{cd} G_{cd}} h^{ab} G_{ab} = T \int \mathrm{d}^2 \sigma \sqrt{-G}.</math>

However, the Polyakov action is more easily quantized because it is linear.

Equations of motionEdit

Using diffeomorphisms and Weyl transformation, with a Minkowskian target space, one can make the physically insignificant transformation <math>\sqrt{-h} h^{ab} \rightarrow \eta^{ab}</math>, thus writing the action in the conformal gauge:

<math> \mathcal{S} = {T \over 2}\int \mathrm{d}^2 \sigma \sqrt{-\eta} \eta^{ab} g_{\mu \nu} (X) \partial_a X^\mu (\sigma) \partial_b X^\nu(\sigma) = {T \over 2}\int \mathrm{d}^2 \sigma \left( \dot{X}^2 - X'^2 \right), </math>

where <math> \eta_{ab} = \left( \begin{array}{cc} 1 & 0 \\ 0 & -1 \end{array} \right) </math>.

Keeping in mind that <math> T_{ab} = 0 </math> one can derive the constraints:

<math>\begin{align}

 T_{01} &= T_{10} = \dot{X} X' = 0, \\
 T_{00} &= T_{11} = \frac12 \left( \dot{X}^2 + X'^2 \right) = 0.

\end{align}</math>

Substituting <math> X^\mu \to X^\mu + \delta X^\mu </math>, one obtains

<math>\begin{align}

 \delta \mathcal{S}
   &= T \int \mathrm{d}^2 \sigma \eta^{ab} \partial_a X^\mu \partial_b \delta X_\mu \\
   &= -T \int \mathrm{d}^2 \sigma \eta^{ab} \partial_a \partial_b X^\mu \delta X_\mu + \left( T \int d \tau X' \delta X \right)_{\sigma=\pi} - \left( T \int d \tau X' \delta X \right)_{\sigma=0} \\
   &= 0.

\end{align}</math>

And consequently

<math> \square X^\mu = \eta^{ab} \partial_a \partial_b X^\mu = 0. </math>

The boundary conditions to satisfy the second part of the variation of the action are as follows.

Closed strings:
Periodic boundary conditions: <math> X^\mu(\tau, \sigma + \pi) = X^\mu(\tau, \sigma). </math>
Open strings:Template:Ordered list

Working in light-cone coordinates <math>\xi^\pm = \tau \pm \sigma</math>, we can rewrite the equations of motion as

<math>\begin{align}

         \partial_+ \partial_- X^\mu &= 0, \\
 (\partial_+ X)^2 = (\partial_- X)^2 &= 0.

\end{align}</math>

Thus, the solution can be written as <math>X^\mu = X^\mu_+ (\xi^+) + X^\mu_- (\xi^-)</math>, and the stress-energy tensor is now diagonal. By Fourier-expanding the solution and imposing canonical commutation relations on the coefficients, applying the second equation of motion motivates the definition of the Virasoro operators and lead to the Virasoro constraints that vanish when acting on physical states.

ReferencesEdit

Template:Reflist

Polyakov action

Contents

Global symmetriesEdit

Local symmetriesEdit

DiffeomorphismsEdit

Weyl transformationEdit

Relation with Nambu–Goto actionEdit

Equations of motionEdit

See alsoEdit

ReferencesEdit

Further readingEdit