Liouville field theory

In physics, Liouville field theory (or simply Liouville theory) is a two-dimensional conformal field theory whose classical equation of motion is a generalization of Liouville's equation.

Liouville theory is defined for all complex values of the central charge $c$ of its Virasoro symmetry algebra, but it is unitary only if $c\in (1,+\infty )$ , and its classical limit is $c\to +\infty$ .

Although it is an interacting theory with a continuous spectrum, Liouville theory has been solved. In particular, its three-point function on the sphere has been determined analytically.

Parameters

Liouville theory has a background charge $Q$ and coupling constant $b$ that are related to the central charge $c$ by

c=1+6Q^{2}\quad ,\quad Q=b+{\frac {1}{b}}\ .

States and fields are characterized by a momentum $\alpha$ that is related to the conformal dimension $\Delta$ by

\Delta =\alpha (Q-\alpha )\ .

The coupling constant and the momentum are the natural parameters for writing correlation functions in Liouville theory. However, the duality

b\to {\frac {1}{b}}\ ,

leaves the central charge invariant, and therefore also leaves the correlation functions invariant. The conformal dimension is invariant under the reflection transformation

\alpha \to Q-\alpha \ ,

and the correlation functions are covariant under reflection.

Spectrum and correlation functions

Spectrum

The spectrum ${\mathcal {S}}$ of Liouville theory is a diagonal combination of Verma modules of the Virasoro algebra,

{\mathcal {S}}=\int _{{\frac {c-1}{24}}+\mathbb {R} _{+}}d\Delta \ {\mathcal {V}}_{\Delta }\otimes {\bar {\mathcal {V}}}_{\Delta }\ ,

where ${\mathcal {V}}_{\Delta }$ and ${\bar {\mathcal {V}}}_{\Delta }$ denote the same Verma module, viewed as a representation of the left- and right-moving Virasoro algebra respectively. In terms of momentums, $\Delta \in {\frac {c-1}{24}}+\mathbb {R} _{+}$ corresponds to $\alpha \in {\frac {Q}{2}}+i\mathbb {R}$ .

Liouville theory is unitary if and only if $c\in (1,+\infty )$ .

The spectrum of Liouville theory does not include a vacuum state. A vacuum state can be defined, but it does not contribute to operator product expansions.

Fields and reflection relation

In Liouville theory, primary fields are usually parametrized by their momentum rather than their conformal dimension, and denoted $V_{\alpha }(z)$ . Both fields $V_{\alpha }(z)$ and $V_{Q-\alpha }(z)$ correspond to the primary state of the representation ${\mathcal {V}}_{\Delta }\otimes {\bar {\mathcal {V}}}_{\Delta }$ , and are related by the reflection relation

V_{\alpha }(z)=R(\alpha )V_{Q-\alpha }(z)\ ,

where the reflection coefficient is^[1]

R(\alpha )=\pm \lambda ^{Q-2\alpha }{\frac {\Gamma (b(2\alpha -Q))\Gamma ({\frac {1}{b}}(2\alpha -Q))}{\Gamma (b(Q-2\alpha ))\Gamma ({\frac {1}{b}}(Q-2\alpha ))}}\ .

(The sign is $+1$ if $c\in (-\infty ,1)$ and $-1$ otherwise, and the normalization parameter $\lambda$ is arbitrary.)

Correlation functions and DOZZ formula

For $c\notin (-\infty ,1)$ , the three-point structure constant is given by the DOZZ formula (for Dorn-Otto^[2] and Zamolodchikov-Zamolodchikov^[3]),

C_{\alpha _{1},\alpha _{2},\alpha _{3}}={\frac {\left[b^{{\frac {2}{b}}-2b}\lambda \right]^{Q-\alpha _{1}-\alpha _{2}-\alpha _{3}}\Upsilon _{b}'(0)\Upsilon _{b}(2\alpha _{1})\Upsilon _{b}(2\alpha _{2})\Upsilon _{b}(2\alpha _{3})}{\Upsilon _{b}(\alpha _{1}+\alpha _{2}+\alpha _{3}-Q)\Upsilon _{b}(\alpha _{1}+\alpha _{2}-\alpha _{3})\Upsilon _{b}(\alpha _{2}+\alpha _{3}-\alpha _{1})\Upsilon _{b}(\alpha _{3}+\alpha _{1}-\alpha _{2})}}\ ,

where the special function $\Upsilon _{b}$ is a kind of multiple gamma function.

For $c\in (-\infty ,1)$ , the three-point structure constant is^[1]

{\hat {C}}_{\alpha _{1},\alpha _{2},\alpha _{3}}={\frac {\left[(ib)^{{\frac {2}{b}}-2b}\lambda \right]^{Q-\alpha _{1}-\alpha _{2}-\alpha _{3}}{\hat {\Upsilon }}_{b}(0){\hat {\Upsilon }}_{b}(2\alpha _{1}){\hat {\Upsilon }}_{b}(2\alpha _{2}){\hat {\Upsilon }}_{b}(2\alpha _{3})}{{\hat {\Upsilon }}_{b}(\alpha _{1}+\alpha _{2}+\alpha _{3}-Q){\hat {\Upsilon }}_{b}(\alpha _{1}+\alpha _{2}-\alpha _{3}){\hat {\Upsilon }}_{b}(\alpha _{2}+\alpha _{3}-\alpha _{1}){\hat {\Upsilon }}_{b}(\alpha _{3}+\alpha _{1}-\alpha _{2})}}\ ,

where

{\hat {\Upsilon }}_{b}(x)={\frac {1}{\Upsilon _{ib}(-ix+ib)}}\ .

$N$ -point functions on the sphere can be expressed in terms of three-point structure constants and conformal blocks. An $N$ -point function may have several different expressions: that they agree is equivalent to crossing symmetry of the four-point function, which has been checked numerically^[3]^[4] and proved analytically.^[5]

Liouville theory exists not only on the sphere, but also on any Riemann surface of genus $g\geq 1$ . Technically, this is equivalent to the modular invariance of the torus one-point function. Due to remarkable identities of conformal blocks and structure constants, this modular invariance property can be deduced from crossing symmetry of the sphere four-point function.^[6]^[4]

Uniqueness of Liouville theory

Using the conformal bootstrap approach, Liouville theory can be shown to be the unique conformal field theory such that^[1]

the spectrum is a continuum, with no multiplicities higher than one,
the correlation functions depend analytically on $b$ and the momentums,
degenerate fields exist.

Lagrangian formulation

Action and equation of motion

Liouville theory is defined by the local action

S[\phi ]={\frac {1}{4\pi }}\int d^{2}x{\sqrt {g}}(g^{\mu \nu }\partial _{\mu }\phi \partial _{\nu }\phi +QR\phi +\lambda 'e^{2b\phi })\ ,

where $g_{{\mu \nu }}$ is the metric of the two-dimensional space on which the theory is formulated, $R$ is the Ricci scalar of that space, and the field $\phi$ is called the Liouville field. The parameter $\lambda '$ , which is sometimes called the cosmological constant, is related to the parameter $\lambda$ that appears in correlation functions by $\lambda '=4{\frac {\Gamma (1-b^{2})}{\Gamma (b^{2})}}\lambda ^{b}$ .

The equation of motion associated to this action is

\Delta \phi (x)={\frac {1}{2}}QR(x)+\lambda 'be^{2b\phi (x)}\ ,

where $\Delta =|g|^{-1/2}\partial _{\mu }(|g|^{1/2}g^{\mu \nu }\partial _{\nu })$ is the Laplace–Beltrami operator. If $g_{{\mu \nu }}$ is the Euclidean metric, this equation reduces to

\left({\frac {\partial ^{2}}{\partial x_{1}^{2}}}+{\frac {\partial ^{2}}{\partial x_{2}^{2}}}\right)\phi (x_{1},x_{2})=\lambda 'be^{2b\phi (x_{1},x_{2})}\ ,

which is equivalent to Liouville's equation.

Conformal symmetry

Using a complex coordinate $z$ and a Euclidean metric $g_{\mu \nu }dx^{\mu }dx^{\nu }=dzd{\bar {z}}$ , the energy-momentum tensor's components obey

T_{z{\bar {z}}}=T_{{\bar {z}}z}=0\quad ,\quad \partial _{\bar {z}}T_{zz}=0\quad ,\quad \partial _{z}T_{{\bar {z}}{\bar {z}}}=0\ .

The non-vanishing components are

T=T_{zz}=(\partial _{z}\phi )^{2}+Q\partial _{z}^{2}\phi \quad ,\quad {\bar {T}}=T_{{\bar {z}}{\bar {z}}}=(\partial _{\bar {z}}\phi )^{2}+Q\partial _{\bar {z}}^{2}\phi \ .

Each one of these two components generates a Virasoro algebra with the central charge $c=1+6Q^{2}$ . For both of these Virasoro algebras, a field $e^{2\alpha \phi }$ is a primary field with the conformal dimension $\Delta =\alpha (Q-\alpha )$ . For the theory to have conformal invariance, the field $e^{2b\phi }$ that appears in the action must be marginal, i.e. have the conformal dimension $\Delta (b)=1$ . This leads to the relation $Q=b+{\frac {1}{b}}$ between the background charge and the coupling constant. If this relation is obeyed, then $e^{2b\phi }$ is actually exactly marginal, and the theory is conformally invariant.

Path integral

The path integral representation of an $N$ -point correlation function of primary fields is

\left\langle \prod _{i=1}^{N}V_{\alpha _{i}}(z_{i})\right\rangle =\int D\phi \ e^{-S[\phi ]}\prod _{i=1}^{N}e^{2\alpha _{i}\phi (z_{i})}\ .

It has been difficult to define and to compute this path integral. In the path integral representation, it is not obvious that Liouville theory has exact conformal invariance, and it is not manifest that correlation functions are invariant under $b\to b^{-1}$ and obey the reflection relation. Nevertheless, the path integral representation can be used for computing the residues of correlation functions at some of their poles as Dotsenko-Fateev integrals (i.e. Coulomb gas integrals), and this is how the DOZZ formula was first guessed in the 1990s. It is only in the 2010s that a rigorous probabilistic construction of the path integral was found, which led to a proof of the DOZZ formula.^[7]

Relations with other conformal field theories

Diagonal minimal models

When the central charge and conformal dimensions are sent to the relevant discrete values, correlation functions of Liouville theory reduce to correlation functions of diagonal (A-series) Virasoro minimal models.^[1]

WZW models

Liouville theory can be obtained from the $SL_{2}(\mathbb {R} )$ Wess–Zumino–Witten model by a quantum Drinfeld-Sokolov reduction. Moreover, correlation functions of the $H_{3}^{+}$ model (the Euclidean version of the $SL_{2}(\mathbb {R} )$ WZW model) can be expressed in terms of correlation functions of Liouville theory.^[8] ^[9] This is also true of correlation functions of the 2d black hole $SL_{2}/U_{1}$ coset model.^[8] Moreover, there exist theories that continuously interpolate between Liouville theory and the $H_{3}^{+}$ model.^[10]

Conformal Toda theory

Liouville theory is the simplest example of a Toda field theory, associated to the $A_{1}$ Cartan matrix. More general conformal Toda theories can be viewed as generalizations of Liouville theory, whose Lagrangians involve several bosons rather than one boson $\phi$ , and whose symmetry algebras are W-algebras rather than the Virasoro algebra.

Supersymmetric Liouville theory

Liouville theory admits two different supersymmetric extensions called ${\mathcal {N}}=1$ supersymmetric Liouville theory and ${\mathcal {N}}=2$ supersymmetric Liouville theory. ^[11].

Applications

Liouville theory appears in the context of string theory when trying to formulate a non-critical version of the theory in the path integral formulation.^[12] Also in the string theory context, if coupled to a free bosonic field, Liouville field theory can be thought of as the theory describing string excitations in a two-dimensional space(time).

Liouville theory is also closely related to other problems in physics and mathematics, like two-dimensional quantum gravity, three-dimensional general relativity in negatively curved spaces, four-dimensional superconformal gauge theories, the uniformization problem of Riemann surfaces, and other problems in conformal mapping. It is also related to instanton partition functions in a certain four-dimensional supersymmetric theory by the AGT correspondence.

References

1 2 3 4 S. Ribault, "Conformal field theory on the plane", arXiv:1406.4290
↑ Dorn, H.; Otto, H.-J. (1992). "On correlation functions for non-critical strings with c⩽1 but d⩾1". Physics Letters B. 291: 39. Bibcode:1992PhLB..291...39D. arXiv:hep-th/9206053 . doi:10.1016/0370-2693(92)90116-L.
1 2 Zamolodchikov, A.; Zamolodchikov, Al. (1996). "Conformal bootstrap in Liouville field theory". Nuclear Physics B. 477 (2): 577. Bibcode:1996NuPhB.477..577Z. arXiv:hep-th/9506136 . doi:10.1016/0550-3213(96)00351-3.
1 2 S. Ribault, R. Santachiara, "Liouville theory with a central charge less than one", arXiv:1503.02067
↑ J. Teschner, "A lecture on the Liouville vertex operators", arXiv:0303150
↑ L. Hadasz, Z. Jaskolski, P. Suchanek, "Modular bootstrap in Liouville field theory", arXiv:0911.4296
↑ A. Kupiainen, R. Rhodes, V. Vargas, "Integrability of Liouville theory: proof of the DOZZ Formula", arXiv:1707.08785
1 2 S. Ribault, J. Teschner, "H(3)+ correlators from Liouville theory", arXiv:hep-th/0502048
↑ Y. Hikida, V. Schomerus, "H^+_3 WZNW model from Liouville field theory",arXiv:0706.1030
↑ S. Ribault, "A family of solvable non-rational conformal field theories",arXiv:0803.2099
↑ Nakayama, Yu (2004). "Liouville Field Theory: A Decade After the Revolution". International Journal of Modern Physics A. 19 (17n18): 2771. Bibcode:2004IJMPA..19.2771N. arXiv:hep-th/0402009 . doi:10.1142/S0217751X04019500.
↑ Polyakov, A.M. (1981). "Quantum geometry of bosonic strings". Physics Letters B. 103 (3): 207. Bibcode:1981PhLB..103..207P. doi:10.1016/0370-2693(81)90743-7.

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