nLab Wess-Zumino-Witten model



\infty-Wess-Zumino-Witten theory

Quantum field theory


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The Wess-Zumino-Witten model (or WZW model for short, also called Wess-Zumino-Novikov-Witten model, or short WZNW model) is a 2-dimensional sigma-model quantum field theory whose target space is a Lie group.

This may be regarded as the boundary theory of Chern-Simons theory for Lie group GG.

The vertex operator algebras corresponding to the WZW model are current algebras.

Action functional

For GG a Lie group, the configuration space of the WZW over a 2-dimensional manifold Σ\Sigma is the space of smooth functions g:ΣGg : \Sigma \to G.

The action functional of the WZW sigma-model is the sum of two terms, a kinetic term and a topological term

S WZW=S kin+S top. S_{WZW} = S_{kin} + S_{top} \,.

Kinetic term

The Lie group canonically carries a Riemannian metric and the kinetic term is the standard one for sigma-models on Riemannian target spaces.

Topological term – WZW term

For the 2d WZW model

In higher differential geometry, then given any closed differential (p+2)-form ωΩ cl p+2(X)\omega \in \Omega^{p+2}_{cl}(X), it is natural to ask for a prequantization of it, namely for a circle (p+1)-bundle with connection \nabla (equivalently: cocycle in degree-(p+2)(p+2)-Deligne cohomology) on XX whose curvature is F =ωF_\nabla = \omega. In terms of moduli stacks this means asking for lifts of the form

B p+1U(1) conn F () X ω Ω cl p+2 \array{ && \mathbf{B}^{p+1}U(1)_{conn} \\ &{}^{\mathllap{\nabla}}\nearrow& \downarrow^{\mathrlap{F_{(-)}}} \\ X &\stackrel{\omega}{\longrightarrow}& \mathbf{\Omega}^{p+2}_{cl} }

in the homotopy theory of smooth homotopy types.

This immediately raises the question for natural classes of examples of such prequantizations.

One such class arises in infinity-Lie theory, where ω\omega is a left invariant form on a smooth infinity-group given by a cocycle in L-infinity algebra cohomology. The prequantum n-bundles arising this way are the higher WZW terms discussed here.

In low degree of traditional Lie theory this appears as follows: On Lie groups GG, those closed (p+2)(p+2)-forms ω\omega which are left invariant forms may be identified, via the general theory of Chevalley-Eilenberg algebras, with degree (p+2)(p+2)-cocycles μ\mu in the Lie algebra cohomology of the Lie algebra 𝔤\mathfrak{g} corresponding to GG. These in turn may arise, via the van Est map, as the Lie differentiation of a degree-(p+2)(p+2)-cocycle c:BGB p+2U(1)\mathbf{c} \colon \mathbf{B}G \to \mathbf{B}^{p+2}U(1) in the Lie group cohomology of GG itself, with coefficients in the circle group U(1)U(1).

This happens to be the case notably for GG a simply connected compact semisimple Lie group such as SU or Spin, where μ=,[,]\mu = \langle -,[-,-]\rangle is the Lie algebra 3-cocycle in transgression with the Killing form invariant polynomial ,\langle -,-\rangle. This is, up to normalization, a representative of the de Rham image of a generator c\mathbf{c} of H 3(BG,U(1))H 4(BG,)H^3(\mathbf{B}G, U(1)) \simeq H^4(B G, \mathbb{Z}) \simeq \mathbb{Z}.

Generally, by the discussion at geometry of physics – principal bundles, the cocycle c\mathbf{c} modulates an infinity-group extension which is a circle p-group-principal infinity-bundle

B pU(1) G^ G Ωc B p+1U(1) \array{ \mathbf{B}^p U(1) &\longrightarrow& \hat G \\ && \downarrow \\ && G &\stackrel{\Omega\mathbf{c}}{\longrightarrow}& \mathbf{B}^{p+1}U(1) }

whose higher Dixmier-Douady class class ΩcH p+2(X,) \int \Omega \mathbf{c} \in H^{p+2}(X,\mathbb{Z}) is an integral lift of the real cohomology class encoded by ω\omega under the de Rham isomorphism. In the example of Spin and p=1p = 1 this extension is the string 2-group.

Such a Lie theoretic situation is concisely expressed by a diagram of smooth homotopy types of the form

B p+1U(1) Ωc θ B pU(1) G ω Ω cl p+2 dRB p+2, \array{ && &\longrightarrow& \mathbf{B}^{p+1}U(1) \\ &{}^{\mathllap{\Omega \mathbf{c}}}\nearrow& &\swArrow_\simeq& \downarrow^{\mathrlap{\theta_{\mathbf{B}^p U(1)}}} \\ G &\stackrel{\omega}{\longrightarrow}& \mathbf{\Omega}_{cl}^{p+2} &\stackrel{}{\longrightarrow}& \flat_{dR}\mathbf{B}^{p+2}\mathbb{R} } \,,

where dRB p+2 dRB p+2U(1)\flat_{dR}\mathbf{B}^{p+2}\mathbb{R} \simeq \flat_{dR}\mathbf{B}^{p+2}U(1) is the de Rham coefficients (see also at geometry of physics – de Rham coefficients) and where the homotopy filling the diagram is what exhibits ω\omega as a de Rham representative of Ωc\Omega \mathbf{c}.

Now, by the very homotopy pullback-characterization of the Deligne complex B p+1U(1) conn\mathbf{B}^{p+1}U(1)_{conn} (here), such a diagram is equivalently a prequantization of ω\omega:

B p+1U(1) conn B p+1U(1) θ B pU(1) G ω Ω cl p+2 dRB p+2. \array{ && \mathbf{B}^{p+1}U(1)_{conn} &\longrightarrow& \mathbf{B}^{p+1}U(1) \\ &{}^\mathllap{\nabla}\nearrow& \downarrow &\swArrow_\simeq& \downarrow^{\mathrlap{\theta_{\mathbf{B}^p U(1)}}} \\ G &\stackrel{\omega}{\longrightarrow}& \mathbf{\Omega}_{cl}^{p+2} &\stackrel{}{\longrightarrow}& \flat_{dR}\mathbf{B}^{p+2}\mathbb{R} } \,.

For ω=,[,]\omega = \langle -,[-,-]\rangle as above, we have p=1p= 1 and so \nabla here is a circle 2-bundle with connection, often referred to as a bundle gerbe with connection. As such, this is also known as the WZW gerbe or similar.

This terminology arises as follows. In (Wess-Zumino 71) the sigma-model for a string propagating on the Lie group GG was considered, with only the standard kinetic action term. Then in (Witten 84) it was observed that for this action functional to give a conformal field theory after quantization, a certain higher gauge interaction term has to the added. The resulting sigma-model came to be known as the Wess-Zumino-Witten model or WZW model for short, and the term that Witten added became the WZW term. In terms of string theory it describes the propagation of the string on the group GG subject to a force of gravity given by the Killing form Riemannian metric and subject to a B-field higher gauge force whose field strength is ω\omega. In (Gawedzki 87) it was observed that when formulated properly and generally, this WZW term is the surface holonomy functional of a connection on a bundle gerbe \nabla on GG. This is equivalently the \nabla that we just motivated above.

Later WZW terms, or at least their curvature forms ω\omega, were recognized all over the place in quantum field theory. For instance the Green-Schwarz sigma-models for super p-branes each have an action functional that is the sum of the standard kinetic action plus a WZW term of degree p+2p+2.

In general WZW terms are “gauged” which means, as we will see, that they are not defined on the give smooth infinity-group GG itself, but on a bundle G˜\tilde G of differential moduli stacks over that group, such that a map ΣG˜\Sigma \to \tilde G is a pair consisting of a map ΣG\Sigma \to G and of a higher gauge field on Σ\Sigma (a “tensor multiplet” of fields).


The following (FSS 12, dcct) is a general axiomatization of WZW terms in cohesive homotopy theory.

In an ambient cohesive (∞,1)-topos H\mathbf{H}, let 𝔾\mathbb{G} be a sylleptic ∞-group, equipped with a Hodge filtration, hence in particular with a chosen morphism

ι:Ω cl 2(,𝔾) dRB 2𝔾 \iota \colon \mathbf{\Omega}^2_{cl}(-,\mathbb{G}) \longrightarrow \flat_{dR} \mathbf{B}^2 \mathbb{G}

to its de Rham coefficients


Given an ∞-group object GG in H\mathbf{H} and given a group cocycle

c:BGB 2𝔾, \mathbf{c} \colon \mathbf{B}G \longrightarrow \mathbf{B}^2 \mathbb{G} \,,

then a refinement of the Hodge filtration of 𝔾\mathbb{G} along c\mathbf{c} is a completion of the cospan formed by dRc\flat_{dR}\mathbf{c} and by ι\iota above to a diagram of the form

Ω flat 1(,G) μ Ω cl 2(,𝔾) ι dRBG dRc dRB 2𝔾. \array{ \mathbf{\Omega}^1_{flat}(-,G) &\stackrel{\mu}{\longrightarrow}& \mathbf{\Omega}^2_{cl}(-,\mathbb{G}) \\ \downarrow && \downarrow^{\mathrlap{\iota}} \\ \flat_{dR}\mathbf{B}G &\stackrel{\flat_{dR}\mathbf{c}}{\longrightarrow}& \flat_{dR}\mathbf{B}^2 \mathbb{G} } \,.

We write G˜\tilde G for the homotopy pullback of this refinement along the Maurer-Cartan form θ G\theta_G of GG

G˜ θ G˜ Ω flat 1(,G) G θ G dRBG. \array{ \tilde G &\stackrel{\theta_{\tilde G}}{\longrightarrow}& \mathbf{\Omega}^1_{flat}(-,G) \\ \downarrow && \downarrow \\ G &\stackrel{\theta_G}{\longrightarrow}& \flat_{dR}\mathbf{B}G } \,.

Let H=\mathbf{H} = Smooth∞Grpd and 𝔾=B pU(1)\mathbb{G} = \mathbf{B}^p U(1) the circle (p+1)-group.

For GG an ordinary Lie group, then μ\mu may be taken to be the Lie algebra cocycle corresponding to c\mathbf{c} and G˜G\tilde G \simeq G.

On the opposite extreme, for G=B pU(1)G = \mathbf{B}^p U(1) itself with c\mathbf{c} the identity, then G˜=B pU(1) conn\tilde G = \mathbf{B}^p U (1)_{conn} is the coefficients for ordinary differential cohomology (the Deligne complex under Dold-Kan correspondence and infinity-stackification).

Hence a more general case is a fibered product of these two, where G˜\tilde G is such that a map ΣG˜\Sigma \longrightarrow \tilde G is equivalently a pair consisting of a map ΣG\Sigma \to G and of differential pp-form data on Σ\Sigma. This is the case of relevance for WZW models of super p-branes with “tensor multiplet” fields on them, such as the D-branes and the M5-brane.


In the situation of def. there is an essentially unique prequantization

L WZW:G˜B 2𝔾 conn \mathbf{L}_{WZW} \colon \tilde G \longrightarrow \mathbf{B}^2 \mathbb{G}_{conn}

of the closed differential form

μ(θ G˜):G˜θ G˜Ω flat 1(,G)μΩ cl 2(,𝔾) \mu(\theta_{\tilde G}) \colon \tilde G \stackrel{\theta_{\tilde G}}{\longrightarrow} \mathbf{\Omega}^1_{flat}(-,G) \stackrel{\mu}{\longrightarrow} \mathbf{\Omega}^2_{cl}(-,\mathbb{G})

whose underlying 𝔾\mathbb{G}-principal ∞-bundle is modulated by the looping Ωc\Omega \mathbf{c} of the original cocycle.

This we call the WZW term of c\mathbf{c} with respect to the chosen refinement of the Hodge structure.


Equations of motion

The variational derivative of the WZW action functional is

δS WZW(g)=k2πi Σ(g 1δg),(g 1¯g). \delta S_{WZW}(g) = -\frac{k}{2 \pi i } \int_\Sigma \langle (g^{-1}\delta g), \partial (g^{-1}\bar \partial g) \rangle \,.

Therefore the classical equations of motion for function g:ΣGg \colon \Sigma \to G are

(g 1¯g)=0¯(gg 1)=0. \partial(g^{-1}\bar \partial g) = 0 \;\;\;\;\;\; \Leftrightarrow \;\;\;\;\;\; \bar \partial(g \partial g^{-1}) = 0 \,.

The space of solutions to these equations is small. However, discussion of the quantization of the theory (below) suggests to consider these equations with the real Lie group GG replaced by its complexification to the complex Lie group G()G({\mathbb{C}}). Then the general solution to the equations of motion above has the form

g(z,z¯)=g (z)g r(z¯) 1 g(z,\bar z) = g_{\ell}(z) g_r(\bar z)^{-1}

where hence g :ΣG()g_{\ell} \colon \Sigma \to G(\mathbb{C}) is any holomorphic function and g rg_r similarly any anti-holomorphic function.

(e.g. Gawedzki 99 (3.18), (3.19))

Holography and Rigorous construction

By the AdS3-CFT2 and CS-WZW correspondence (see there for more details) the 2d WZW CFT on GG is related to GG-Chern-Simons theory in 3d3d.

In fact a rigorous constructions of the GG-WZW model as a rational 2d CFT is via the FRS-theorem on rational 2d CFT, which constructs the model as a boundary field theory of the GG-Chern-Simons theory as a 3d TQFT incarnated via a Reshetikhin-Turaev construction.

Braid representations via twisted cohomology of configuration spaces

The “hypergeometric integral” construction of conformal blocks for affine Lie algebra/WZW model-2d CFTs and of more general solutions to the Knizhnik-Zamolodchikov equation, via twisted de Rham cohomology of configuration spaces of points, originates with:

following precursor observations due to:

The proof that for rational levels this construction indeed yields conformal blocks is due to:


See also:

This “hypergeometric” construction uses results on the twisted de Rham cohomology of configuration spaces of points due to:


reviewed in:

  • Yukihito Kawahara, The twisted de Rham cohomology for basic constructions of hyperplane arrangements and its applications, Hokkaido Math. J. 34 2 (2005) 489-505 [[doi:10.14492/hokmj/1285766233]]

Discussion for the special case of level=0=0 (cf. at logarithmic CFT – Examples):

Interpretation of the hypergeometric construction as happening in twisted equivariant differential K-theory, showing that the K-theory classification of D-brane charge and the K-theory classification of topological phases of matter both reflect braid group representations as expected for defect branes and for anyons/topological order, respectively:

D-branes for the WZW model

The characterization of D-brane submanifolds for the open string WZW model on a Lie group GG comes from two consistency conditions:

  1. geometrical condition:

    For the open string CFT to still have current algebra worldsheet symmetry, hence for half the current algebra symmetry of the closed WZW string to be preserved, the D-brane submanifolds need to be conjugacy classes of the group manifold (see e.g. Alekseev-Schomerus for a brief review and further pointers). These conjugacy classes are therefore also called the symmetric D-branes.

    Notice that these conjugacy classes are equivalently the leaves of the foliation induced by the canonical Cartan-Dirac structure on GG, hence (by the discussion at Dirac structure), the leaves induced by the Lagrangian sub-Lie 2-algebroids of the Courant Lie 2-algebroid which is the higher gauge groupoid (see there) of the background B-field on GG.(It has been suggested by Chris Rogers that such a foliation be thought of as a higher real polarization.)

  2. cohomological condition:

    In order for the Kapustin-part of the Freed-Witten-Kapustin anomaly of the worldsheet action functional of the open WZW string to vanish, the D-brane must be equipped with a Chan-Paton gauge field, hence a twisted unitary bundle (bundle gerbe module) of some rank nn \in \mathbb{N} for the restriction of the ambient B-field to the brane.

    For simply connected Lie groups only the rank-1 Chan-Paton gauge fields and their direct sums play a role, and their existence corresponds to a trivialization of the underlying BU(1)\mathbf{B}U(1)-principal 2-bundle (U(1)U(1)-bundle gerbe) of the restriction of the B-field to the brane. There is then a discrete finite collection of symmetric D-branes = conjugacy classes satisfying this condition, and these are called the integral symmetric D-branes. (Alekseev-Schomerus, Gawedzki-Reis). As observed in Alekseev-Schomerus, this may be thought of as identifying a D-brane as a variant kind of a Bohr-Sommerfeld leaf.

    More generally, on non-simply connected group manifolds there are nontrivial higher rank twisted unitary bundles/Chan-Paton gauge fields over conjugacy classes and hence the cohomological “integrality” or “Bohr-Sommerfeld”-condition imposed on symmetric D-branes becomes more refined (Gawedzki 04).

In summary, the D-brane submanifolds in a Lie group which induce an open string WZW model that a) has one current algebra symmetry and b) is Kapustin-anomaly-free are precisely the conjugacy class-submanifolds GG equipped with a twisted unitary bundle for the restriction of the background B-field to the conjugacy class.


on quantization of the WZW model, see at


Introduction and survey

Textbook accounts:

Lecture notes:

A basic introduction also to the super-WZW model (and with an eye towards the corresponding 2-spectral triple) is in

A useful account of the WZW model that encompasses both its action functional and path integral quantization as well as the current algebra aspects of the QFT is in

This starts in section 2 as a warmup with describing the 1d QFT of a particle propagating on a group manifold. The Hilbert space of states is expressed in terms of the Lie theory of GG and its Lie algebra 𝔤\mathfrak{g}.

In section 4 the quantization of the 2d WZW model is discussed in analogy to that. In lack of a full formalization of the quantization procedure, the author uses the loop algebra 𝓁𝔤\mathcal{l} \mathfrak{g} – the affine Lie algebra – of 𝔤\mathfrak{g} as the evident analog that replaces 𝔤\mathfrak{g} and discusses the Hilbert space of states in terms of that. He also indicates how this may be understood as a space of sections of a (prequantum) line bundle over the loop group.

See also

The WZW term of QCD chiral perturbation theory

The gauged WZW term of chiral perturbation theory/quantum hadrodynamics which reproduces the chiral anomaly of QCD in the effective field theory of mesons and Skyrmions:


The original articles:

See also:

  • O. Kaymakcalan, S. Rajeev, J. Schechter, Nonabelian Anomaly and Vector Meson Decays, Phys. Rev. D 30 (1984) 594 (spire:194756)

Corrections and streamlining of the computations:

  • Chou Kuang-chao, Guo Han-ying, Wu Ke, Song Xing-kang, On the gauge invariance and anomaly-free condition of the Wess-Zumino-Witten effective action, Physics Letters B Volume 134, Issues 1–2, 5 January 1984, Pages 67-69 (doi:10.1016/0370-2693(84)90986-9))

  • H. Kawai, S.-H. H. Tye, Chiral anomalies, effective lagrangians and differential geometry, Physics Letters B Volume 140, Issues 5–6, 14 June 1984, Pages 403-407 (doi:10.1016/0370-2693(84)90780-9)

  • J. L. Mañes, Differential geometric construction of the gauged Wess-Zumino action, Nuclear Physics B Volume 250, Issues 1–4, 1985, Pages 369-384 (doi:10.1016/0550-3213(85)90487-0)

  • Tomáš Brauner, Helena Kolešová, Gauged Wess-Zumino terms for a general coset space, Nuclear Physics B Volume 945, August 2019, 114676 (doi:10.1016/j.nuclphysb.2019.114676)

See also

Interpretation as Skyrmion/baryon current:

Concrete form for NN-flavor quantum hadrodynamics in 2d:

  • C. R. Lee, H. C. Yen, A Derivation of The Wess-Zumino-Witten Action from Chiral Anomaly Using Homotopy Operators, Chinese Journal of Physics, Vol 23 No. 1 (1985) (spire:16389, pdf)

Concrete form for 2 flavors in 4d:

  • Masashi Wakamatsu, On the electromagnetic hadron current derived from the gauged Wess-Zumino-Witten action, (arXiv:1108.1236, spire:922302)

Including light vector mesons

Concrete form for 2-flavor quantum hadrodynamics in 4d with light vector mesons included (omega-meson and rho-meson):

Including heavy scalar mesons

Including heavy scalar mesons:

specifically kaons:

specifically D-mesons:


specifically B-mesons:

  • Mannque Rho, D. O. Riska, N. N. Scoccola, above (2.1) in: The energy levels of the heavy flavour baryons in the topological soliton model, Zeitschrift für Physik A Hadrons and Nuclei volume 341, pages343–352 (1992) (doi:10.1007/BF01283544)

Including heavy vector mesons

Inclusion of heavy vector mesons:

specifically K*-mesons:

Including electroweak interactions

Including electroweak fields:

Discussion for the full standard model of particle physics:

  • Jeffrey Harvey, Christopher T. Hill, Richard J. Hill, Standard Model Gauging of the WZW Term: Anomalies, Global Currents and pseudo-Chern-Simons Interactions, Phys. Rev. D77:085017, 2008 (arXiv:0712.1230)

Interpretation via CFT and gerbes

Interpretation of the 3d WZW term as defining a 2d CFT

and hence as part of a perturbative string theory vacuum/target space

The WZ term on Σ 2\Sigma_2 was understood in terms of an integral of a 3-form over a cobounding manifold Σ 3\Sigma_3 in

for the case that Σ 2\Sigma_2 is closed, and generally, in terms of surface holonomy of bundle gerbes/circle 2-bundles with connection in

  • Krzysztof Gawedzki, Topological Actions in two-dimensional Quantum Field Theories, in Gerard 't Hooft et. al (eds.) Nonperturbative quantum field theory Cargese 1987 proceedings, (web)

  • Giovanni Felder , Krzysztof Gawedzki, A. Kupianen, Spectra of Wess-Zumino-Witten models with arbitrary simple groups. Commun. Math. Phys. 117, 127 (1988)

  • Krzysztof Gawedzki, Topological actions in two-dimensional quantum field theories. In: Nonperturbative quantum field theory. ‘tHooft, G. et al. (eds.). London: Plenum Press 1988

as the surface holonomy of a circle 2-bundle with connection. See also the references at B-field and at Freed-Witten anomaly cancellation.

See also

For the fully general understanding as the surface holonomy of a circle 2-bundle with connection see the references below.

See also

  • Edward Witten, On holomorphic factorization of WZW and coset models, Comm. Math. Phys. Volume 144, Number 1 (1992), 189-212. (Euclid)

Relation to gerbes and Chern-Simons theory

Discussion of circle 2-bundles with connection (expressed in terms of bundle gerbes) and discussion of the WZW-background B-field (WZW term) in this language (cf. basic bundle gerbe)

Discussion of how this 2-bundle arises from the Chern-Simons circle 3-bundle is in

and related discussion is in

See also Section 2.3.18 and section 4.7 of

Partition functions

D-branes for the WZW model

A characterization of D-branes in the WZW model as those conjugacy classes that in addition satisfy an integrality (Bohr-Sommerfeld-type) condition missed in other parts of the literature is stated in

The refined interpretation of the integrality condition as a choice of trivialization of the underling principal 2-bundle/bundle gerbe of the B-field over the brane was then noticed in section 7 of

The observation that this is just the special rank-1 case of the more general structure provided by a twisted unitary bundle of some rank nn on the D-brane (gerbe module) which is twisted by the restriction of the B-field to the D-brane – the Chan-Paton gauge field – is due to

The observation that the “multiplicative” structure of the WZW-B-field (induced from it being the transgression of the Chern-Simons circle 3-connection over the moduli stack of GG-principal connections) induces the Verlinde ring fusion product structure on symmetric D-branes equipped with Chan-Paton gauge fields is discussed in

The image in K-theory of these Chan-Paton gauge fields over conjugacy classes is shown to generate the Verlinde ring/the positive energy representations of the loop group in

Formalization of WZW terms in cohesive homotopy theory is in

Relation to dimensional reduction of Chern-Simons

One can also obtain the WZW-model by KK-reduction from Chern-Simons theory.


A discussion in higher differential geometry via transgression in ordinary differential cohomology is in

Relation to extended TQFT

Relation to extended TQFT is discussed in

For a formulation of the WZW term in the presence of D-branes as an open-closed smooth functorial field theory:

The formulation of the Green-Schwarz action functional for superstrings (and other branes of string theory/M-theory) as WZW-models (and ∞-WZW models) on (super L-∞ algebra L-∞ extensions of) the super translation group is in

In solid state physics

The low-energy physics of a Heisenberg antiferromagnetic spin chain is argued to be described by a WZW model in

  • Zheng-Xin Liu, Guang-Ming Zhang, Classification of quantum critical states of integrable antiferromagnetic spin chains and their correspondent two-dimensional topological phases (arXiv:1211.5421)

See also section 7.10 of Fradkin’s book.

Discussion of symmetry protected topological order phases of matter in solid state physics via higher dimensional WZW models is in

  • Xie Chen, Zheng-Cheng Gu, Zheng-Xin Liu, Xiao-Gang Wen, Symmetry protected topological orders and the group cohomology of their symmetry group, Phys. Rev. B 87, 155114 (2013) arXiv:1106.4772; A short version in Science 338, 1604-1606 (2012) pdf

On fractional-level WZW models as logarithmic CFTs

On WZW models at fractional level:

with a good review in:

On braided fusion categories formed by affine Lie algebra-representations at admissible fractional level:

On interpreting fractional level WZW models as logarithmic CFTs:

Reviewed in:

In particular, the logarithmic c=2c = -2 model is essentially an admissible-level WZW model (namely at level k=0k = 0):

with a comprehensive account in:

On the c=1c = -1 model as the 𝔰𝔲(2)\mathfrak{su}(2) WZW model at fractional level 1/2-1/2 and relation to the beta-gamma system:

and its lift to a logarithmic CFT:

  • F. Lesage, P. Mathieu, J. Rasmussen, H. Saleur, Logarithmic lift of the 𝔰𝔲(2) 1/2\mathfrak{su}(2)_{-1/2} model, Nuclear Physics B 686 3 (2004) 313-346 [doi:10.1016/j.nuclphysb.2004.02.039]

On quasi-characters at fractional level:

Identification of would-be fractional level 𝔰𝔲 ( 2 ) \mathfrak{su}(2) conformal blocks in twisted equivariant K-theory of configuration spaces of points:

Last revised on December 2, 2023 at 11:45:04. See the history of this page for a list of all contributions to it.