W-algebra

For W*-algebra, see Von Neumann algebra.

In conformal field theory and representation theory, a W-algebra is an associative algebra that generalizes the Virasoro algebra. W-algebras were introduced by Alexander Zamolodchikov, ^[1] and the name "W-algebra" comes from the fact that Zamolodchikov used the letter W for one of the elements of one of his examples.

Definition

A W-algebra is an associative algebra that is generated by the modes of a finite number of meromorphic fields ${\displaystyle W^{(h)}(z)}$, including the energy-momentum tensor ${\displaystyle T(z)=W^{(2)}(z)}$. For ${\displaystyle h\neq 2}$, ${\displaystyle W^{(h)}(z)}$ is a primary field of conformal dimension ${\displaystyle h\in {\frac {1}{2}}\mathbb {N} ^{*}}$. ^[2] The generators ${\displaystyle (W_{n}^{(h)})_{n\in \mathbb {Z} }}$ of the algebra are related to the meromorphic fields by the mode expansions

${\displaystyle W^{(h)}(z)=\sum _{n\in \mathbb {Z} }W_{n}^{(h)}z^{-n-h}}$

The commutation relations of ${\displaystyle L_{n}=W_{n}^{(2)}}$ are given by the Virasoro algebra, which is parameterized by a central charge ${\displaystyle c\in \mathbb {C} }$. This number is also called the central charge of the W-algebra. The commutation relations

${\displaystyle [L_{m},W_{n}^{(h)}]=((h-1)m-n)W_{m+n}^{(h)}}$

are equivalent to the assumption that ${\displaystyle W^{(h)}(z)}$ is a primary field of dimension ${\displaystyle h}$. The rest of the commutation relations can in principle be determined by solving the Jacobi identities.

Given a finite set of conformal dimensions ${\displaystyle H}$ (not necessarily all distinct), the number of W-algebras generated by ${\displaystyle (W^{(h)})_{h\in H}}$ may be zero, one or more. The resulting W-algebras may exist for all ${\displaystyle c\in \mathbb {C} }$, or only for some specific values of the central charge. ^[2]

A W-algebra is called freely generated if its generators obey no other relations than the commutation relations. Most commonly studied W-algebras are freely generated, including the W(N) algebras. ^[3] In this article, the sections on representation theory and correlation functions apply to freely generated W-algebras.

Constructions

While it is possible to construct W-algebras by assuming the existence of a number of meromorphic fields ${\displaystyle W^{(h)}(z)}$ and solving the Jacobi identities, there also exist systematic constructions of families of W-algebras.

Drinfeld-Sokolov reduction

From a finite-dimensional Lie algebra ${\displaystyle {\mathfrak {g}}}$, together with an embedding ${\displaystyle {\mathfrak {sl}}_{2}\hookrightarrow {\mathfrak {g}}}$, a W-algebra may be constructed from the universal enveloping algebra of the affine Lie algebra ${\displaystyle {\hat {\mathfrak {g}}}}$ by a kind of BRST construction. ^[2] Then the central charge of the W-algebra is a function of the level of the affine Lie algebra.

Coset construction

Given a finite-dimensional Lie algebra ${\displaystyle {\mathfrak {g}}}$, together with a subalgebra ${\displaystyle {\mathfrak {h}}\hookrightarrow {\mathfrak {g}}}$, a W-algebra ${\displaystyle W({\hat {\mathfrak {g}}}/{\hat {\mathfrak {h}}})}$ may be constructed from the corresponding affine Lie algebras ${\displaystyle {\hat {\mathfrak {h}}}\hookrightarrow {\hat {\mathfrak {g}}}}$. The fields that generate ${\displaystyle W({\hat {\mathfrak {g}}}/{\hat {\mathfrak {h}}})}$ are the polynomials in the currents of ${\displaystyle {\hat {\mathfrak {g}}}}$ and their derivatives that commute with the currents of ${\displaystyle {\hat {\mathfrak {h}}}}$. ^[2] The central charge of ${\displaystyle W({\hat {\mathfrak {g}}}/{\hat {\mathfrak {h}}})}$ is the difference of the central charges of ${\displaystyle {\hat {\mathfrak {g}}}}$ and ${\displaystyle {\hat {\mathfrak {h}}}}$, which are themselves given in terms of their level by the Sugawara construction.

Commutator of a set of screenings

Given a holomorphic field ${\displaystyle \phi (z)}$ with values in ${\displaystyle \mathbb {R} ^{n}}$, and a set of ${\displaystyle n}$ vectors ${\displaystyle a_{1},\dots ,a_{n}\in \mathbb {R} ^{n}}$, a W-algebra may be defined as the set of polynomials of ${\displaystyle \phi }$ and its derivatives that commute with the screening charges ${\displaystyle \oint e^{(a_{i},\phi (z))}dz}$. If the vectors ${\displaystyle a_{i}}$ are the simple roots of a Lie algebra ${\displaystyle {\mathfrak {g}}}$, the resulting W-algebra coincides with an algebra that is obtained from ${\displaystyle {\mathfrak {g}}}$ by Drinfeld-Sokolov reduction. ^[4]

The W(N) algebras

For any integer ${\displaystyle N\geq 2}$, the W(N) algebra is a W-algebra which is generated by ${\displaystyle N-1}$ meromorphic fields of dimensions ${\displaystyle 2,3,\dots ,N}$. The W(2) algebra coincides with the Virasoro algebra.

Construction

The W(N) algebra is obtained by Drinfeld-Sokolov reduction of the affine Lie algebra ${\displaystyle {\widehat {\mathfrak {sl}}}_{N}}$.

The embeddings ${\displaystyle {\mathfrak {sl}}_{2}\hookrightarrow {\mathfrak {sl}}_{N}}$ are parametrized by the integer partitions of ${\displaystyle N}$, interpreted as decompositions of the fundamental representation ${\displaystyle F}$ of ${\displaystyle {\mathfrak {sl}}_{N}}$ into representations of ${\displaystyle {\mathfrak {sl}}_{2}}$. The set ${\displaystyle H}$ of dimensions of the generators of the resulting W-algebra is such that ${\displaystyle F\otimes F=R_{1}\oplus \bigoplus _{h\in H}R_{2h-1}}$ where ${\displaystyle R_{d}}$ is the ${\displaystyle d}$-dimensional irreducible representation of ${\displaystyle {\mathfrak {sl}}_{2}}$. ^[5]

The trivial partition ${\displaystyle N=N}$ corresponds to the W(N) algebra, while ${\displaystyle N=1+1+\dots +1}$ corresponds to ${\displaystyle {\widehat {\mathfrak {sl}}}_{N}}$ itself. In the case ${\displaystyle N=3}$, the partition ${\displaystyle 3=2+1}$ leads to the Bershadsky-Polyakov algebra, whose generating fields have the dimensions ${\displaystyle 2,{\frac {3}{2}},{\frac {3}{2}},1}$.

Properties

The central charge of the W(N) algebra is given in terms of the level ${\displaystyle k}$ of the affine Lie algebra by

${\displaystyle c_{W(N)}=(N-1)\left(1-N(N+1)\left({\frac {1}{k+N}}+k+N-2\right)\right)}$

in notations where the central charge of the affine Lie algebra is

${\displaystyle c_{{\widehat {\mathfrak {sl}}}_{N}}=(N-1)(N+1)-{\frac {N(N-1)(N+1)}{k+N}}}$

It is possible to choose a basis such that the commutation relations are invariant under ${\displaystyle W^{(h)}\to (-1)^{h}W^{(h)}}$.

While the Virasoro algebra is a subalgebra of the universal enveloping algebra of ${\displaystyle {\widehat {\mathfrak {sl}}}_{2}}$, the W(N) algebra with ${\displaystyle N\geq 3}$ is not a subalgebra of the universal enveloping algebra of ${\displaystyle {\widehat {\mathfrak {sl}}}_{N}}$. ^[6]

Example of the W(3) algebra

The W(3) algebra is generated by the generators of the Virasoro algebra ${\displaystyle (L_{n})_{n\in \mathbb {Z} }}$, plus another infinite family of generators ${\displaystyle (W_{n})_{n\in \mathbb {Z} }=(W_{n}^{(3)})_{n\in \mathbb {Z} }}$. The commutation relations are ^[2]

${\displaystyle [L_{m},L_{n}]=(m-n)L_{m+n}+{\frac {c}{12}}m(m^{2}-1)\delta _{m+n,0}}$

${\displaystyle [L_{m},W_{n}]=(2m-n)W_{m+n}}$

${\displaystyle [W_{m},W_{n}]={\frac {c}{360}}m(m^{2}-1)(m^{2}-4)\delta _{m+n,0}+{\frac {16}{22+5c}}\Lambda _{m+n}+{\frac {(m-n)(2m^{2}-mn+2n^{2}-8)}{30}}L_{m+n}}$

where ${\displaystyle c\in \mathbb {C} }$ is the central charge, and we define

${\displaystyle \Lambda _{n}=\sum _{m=-\infty }^{-2}L_{m}L_{n-m}+\sum _{m=-1}^{\infty }L_{n-m}L_{m}-{\frac {3}{10}}(n+2)(n+3)L_{n}}$

The field ${\displaystyle \Lambda (z)=\sum _{n\in \mathbb {Z} }\Lambda _{n}z^{-n-4}}$ is such that ${\displaystyle \Lambda =(TT)-{\frac {3}{10}}T''}$.

Representation theory

Highest weight representations

A highest weight representation of a W-algebra is a representation that is generated by a primary state: a vector ${\displaystyle v}$ such that

${\displaystyle W_{n>0}^{(h)}v=0\quad ,\quad W_{0}^{(h)}v=q^{(h)}v}$

for some numbers ${\displaystyle q^{(h)}}$ called the charges, including the conformal dimension ${\displaystyle q^{(2)}=\Delta }$.

Given a set ${\displaystyle {\vec {q}}=(q^{(h)})_{h\in H}}$ of charges, the corresponding Verma module is the largest highest-weight representation that is generated by a primary state with these charges. A basis of the Verma module is

${\displaystyle \left\{\prod _{h\in H}W_{-{\vec {N}}_{h}}^{(h)}v\right\}_{{\vec {N}}_{h}\in {\mathcal {V}}}}$

where ${\displaystyle {\mathcal {V}}}$ is the set of ordered tuples of strictly positive integers of the type ${\displaystyle {\vec {N}}=(n_{1},n_{2},\dots ,n_{p})}$ with ${\displaystyle 0<n_{1}\leq n_{2}\leq \dots \leq n_{p}}$, and ${\displaystyle W_{-{\vec {N}}}=W_{-n_{1}}W_{-n_{2}}\dots W_{-n_{p}}}$. Except for ${\displaystyle v}$ itself, the elements of this basis are called descendant states, and their linear combinations are also called descendant states.

For generic values of the charges, the Verma module is the only highest weight representation. For special values of the charges that depend on the algebra's central charge, there exist other highest weight representations, called degenerate representations. Degenerate representations exist if the Verma module is reducible, and they are quotients of the Verma module by its nontrivial submodules.

Degenerate representations

If a Verma module is reducible, any indecomposible submodule is itself a highest weight representation, and is generated by a state that is both descendant and primary, called a null state or null vector. A degenerate representation is obtained by setting one or more null vectors to zero. Setting all the null vectors to zero leads to an irreducible representation.

The structures and characters of irreducible representations can be deduced by Drinfeld-Sokolov reduction from representations of affine Lie algebras. ^[7]

The existence of null vectors is possible only under ${\displaystyle c}$-dependent constraints on the charge ${\displaystyle {\vec {q}}}$. A Verma module can have only finitely many null vectors that are not descendants of other null vectors. If we start from a Verma module that has a maximal number of null vectors, and set all these null vectors to zero, we obtain an irreducible representation called a fully degenerate representation.

For example, in the case of the algebra W(3), the Verma module with vanishing charges ${\displaystyle q^{(2)}=q^{(3)}=0}$ has the three null vectors ${\displaystyle L_{-1}v,W_{-1}v,W_{-2}v}$ at levels 1, 1 and 2. Setting these null vectors to zero yields a fully degenerate representation called the vacuum module. The simplest nontrivial fully degenerate representation of W(3) has vanishing null vectors at levels 1, 2 and 3, whose expressions are explicitly known. ^[8]

An alternative characterization of a fully degenerate representation is that its fusion product with any Verma module is a sum of finitely many indecomposable representations. ^[8]

Case of W(N)

It is convenient to parametrize highest-weight representations not by the set of charges ${\displaystyle {\vec {q}}=(q^{(2)},\dots ,q^{(N)})}$, but by an element ${\displaystyle P}$ of the weight space of ${\displaystyle {\mathfrak {sl}}_{N}}$, called the momentum.

Let ${\displaystyle e_{1},\dots ,e_{N-1}}$ be the simple roots of ${\displaystyle {\mathfrak {sl}}_{N}}$, with a scalar product ${\displaystyle K_{ij}=(e_{i},e_{j})}$ given by the Cartan matrix of ${\displaystyle {\mathfrak {sl}}_{N}}$, whose nonzero elements are ${\displaystyle K_{ii}=2,K_{i,i+1}=K_{i,i-1}=-1}$. The ${\displaystyle {\frac {1}{2}}N(N-1)}$ positive simple roots are sums of any number of consecutive simple roots, and the Weyl vector is their half-sum ${\displaystyle \rho ={\frac {1}{2}}\sum _{e>0}e}$, which obeys ${\displaystyle (\rho ,\rho )={\frac {1}{12}}N(N^{2}-1)}$. The fundamental weights ${\displaystyle \omega _{1},\dots ,\omega _{N-1}}$ are defined by ${\displaystyle (\omega _{i},e_{j})=\delta _{ij}}$. Then the momentum is a vector

${\displaystyle P=\sum _{i=1}^{N-1}P_{i}\omega _{i}\quad i.e.\quad (e_{i},P)=P_{i}}$

The charges ${\displaystyle q^{(h)}}$ are functions of the momentum and the central charge, invariant under the action of the Weyl group. In particular, ${\displaystyle q^{(h)}}$ is a polynomial of the momentum of degree ${\displaystyle h}$, which under the Dynkin diagram automorphism ${\displaystyle e_{i}^{*}=e_{N-i}}$ behaves as ${\displaystyle q^{(h)}(P^{*})=(-1)^{h}q^{(h)}(P)}$. The conformal dimension is ^[9]

${\displaystyle q^{(2)}={\frac {c+1-N}{24}}-(P,P)}$

Let us parametrize the central charge in terms of a number ${\displaystyle b}$ such that

${\displaystyle c=(N-1){\big (}1+N(N+1)\left(b+b^{-1}\right)^{2}{\big )}}$

If there is a positive root ${\displaystyle e>0}$ and two integers ${\displaystyle r,s\in \mathbb {N} ^{*}}$ such that ^[9]

${\displaystyle (e,P)=rb+sb^{-1}}$

then the Verma module of momentum ${\displaystyle P}$ has a null vector at level ${\displaystyle rs}$. This null vector is itself a primary state of momentum ${\displaystyle P-rbe}$ or equivalently (by a Weyl reflection) ${\displaystyle P-sb^{-1}e}$. The number of independent null vectors is the number of positive roots such that ${\displaystyle (e,P)\in \mathbb {N} ^{*}b+\mathbb {N} ^{*}b^{-1}}$ (up to a Weyl reflection).

The maximal number of null vectors is the number of positive roots ${\displaystyle {\frac {1}{2}}N(N-1)}$. The corresponding momentums are of the type ^[9]

${\displaystyle P=(b+b^{-1})\rho +b\Omega ^{+}+b^{-1}\Omega ^{-}}$

where ${\displaystyle \Omega ^{+},\Omega ^{-}}$ are integral dominant weights, i.e. elements of ${\displaystyle \sum _{i=1}^{N-1}\mathbb {N} \omega _{i}}$, which are highest weights of irreducible finite-dimensional representations of ${\displaystyle {\mathfrak {sl}}_{N}}$. Let us call ${\displaystyle {\mathcal {R}}_{\Omega _{+},\Omega _{-}}}$ the corresponding fully degenerate representation of the W(N) algebra.

The irreducible finite-dimensional representation ${\displaystyle R_{\Omega }}$ of ${\displaystyle {\mathfrak {sl}}_{N}}$ of highest weight ${\displaystyle \Omega }$ has a finite set of weights ${\displaystyle \Lambda _{\Omega }}$, with ${\displaystyle |\Lambda _{\Omega }|=\dim(R_{\Omega })}$. Its tensor product with a Verma module ${\displaystyle V_{p}}$ of weight ${\displaystyle p\in \sum _{i=1}^{N-1}\mathbb {R} \omega _{i}}$ is ${\displaystyle R_{\Omega }\otimes V_{p}=\bigoplus _{\lambda \in \Lambda _{\Omega }}V_{p+\lambda }}$. The fusion product of the fully degenerate representation ${\displaystyle {\mathcal {R}}_{\Omega _{+},\Omega _{-}}}$ of W(N) with a Verma module ${\displaystyle {\mathcal {V}}_{P}}$ of momentum ${\displaystyle P}$ is then

${\displaystyle {\mathcal {R}}_{\Omega _{+},\Omega _{-}}\times {\mathcal {V}}_{P}=\sum _{\lambda _{+}\in \Lambda _{\Omega _{+}}}\sum _{\lambda _{-}\in \Lambda _{\Omega _{-}}}{\mathcal {V}}_{P+b\lambda _{+}+b^{-1}\lambda _{-}}}$

Correlation functions

Primary fields

To a primary state of charge ${\displaystyle {\vec {q}}=(q^{(h)})_{h\in H}}$, the state-field correspondence associates a primary field ${\displaystyle V_{\vec {q}}(z)}$, whose operator product expansions with the fields ${\displaystyle W^{(h)}(z)}$ are

${\displaystyle W^{(h)}(y)V_{\vec {q}}(z)=\left({\frac {q^{(h)}}{(y-z)^{h}}}+\sum _{n=1}^{h-1}{\frac {W_{-n}^{(h)}}{(y-z)^{h-n}}}\right)V_{\vec {q}}(z)+O(1)}$

On any field ${\displaystyle V(z)}$, the mode ${\displaystyle L_{-1}}$ of the energy-momentum tensor acts as a derivative, ${\displaystyle L_{-1}V(z)={\frac {\partial }{\partial z}}V(z)}$.

Ward identities

On the Riemann sphere, if there is no field at infinity, we have ${\displaystyle W^{(h)}(y){\underset {y\to \infty }{=}}O\left(y^{-2h}\right)}$. For ${\displaystyle n=0,1,\dots ,2h-2}$, the identity ${\displaystyle \oint _{\infty }dy\ y^{n}W^{(h)}(y)=0}$ may be inserted in any correlation function. Therefore, the field ${\displaystyle W^{(h)}(y)}$ gives rise to ${\displaystyle 2h-1}$ global Ward identities.

Local Ward identities are obtained by inserting ${\displaystyle \oint _{\infty }dy\ \varphi (y)W^{(h)}(y)=0}$, where ${\displaystyle \varphi (y)}$ is a meromorphic function such that ${\displaystyle \varphi (y){\underset {y\to \infty }{=}}O\left(y^{2h-2}\right)}$. In a correlation function of primary fields, local Ward identities determine the action of ${\displaystyle W_{-n}^{(h)}}$ with ${\displaystyle n\geq h}$ in terms of the action of ${\displaystyle W_{-n}^{(h)}}$ with ${\displaystyle n\leq h-1}$.

For example, in the case of a three-point function on the sphere ${\displaystyle \left\langle \prod _{i=1}^{3}V_{{\vec {q}}_{i}}(z_{i})\right\rangle }$ of W(3)-primary fields, local Ward identities determine all the descendant three-point functions as linear combinations of descendant three-point functions that involve only ${\displaystyle L_{-1},W_{-1},W_{-2}}$. Global Ward identities further reduce the problem to determining three-point functions of the type ${\displaystyle \left\langle V_{{\vec {q}}_{1}}(z_{1})V_{{\vec {q}}_{2}}(z_{2})W_{-1}^{k}V_{{\vec {q}}_{3}}(z_{3})\right\rangle }$ for ${\displaystyle k\in \mathbb {N} }$.

In the W(3) algebra, as in generic W-algebras, correlation functions of descendant fields can therefore not be deduced from correlation functions of primary fields using Ward identities, as was the case for the Virasoro algebra. A W(3)-Verma module appears in the fusion product of two other W(3)-Verma modules with a multiplicity that is in general infinite.

Differential equations

A correlation function may obey a differential equation that generalizes the BPZ equations if the fields have sufficiently many vanishing null vectors.

A four-point function of W(N)-primary fields on the sphere with one fully degenerate field obeys a differential equation if ${\displaystyle N=2}$ but not if ${\displaystyle N\geq 3}$. In the latter case, for a differential equation to exist, one of the other fields must have vanishing null vectors. For example, a four-point function with two fields of momentums ${\displaystyle P_{1}=(b+b^{-1})\rho +b\omega _{1}}$ (fully degenerate) and ${\displaystyle P_{2}=(b+b^{-1})\rho +x\omega _{N-1}}$ with ${\displaystyle x\in \mathbb {C} }$ (almost fully degenerate) obeys a differential equation whose solutions are generalized hypergeometric functions of type ${\displaystyle {}_{N}F_{N-1}}$. ^[10]

Applications to conformal field theory

W-minimal models

W-minimal models are generalizations of Virasoro minimal models based on a W-algebra. Their spaces of states are made of finitely many fully degenerate representations. They exist for certain rational values of the central charge: in the case of the W(N) algebra, values of the type

${\displaystyle c_{p,q}^{(N)}=N-1-N(N^{2}-1){\frac {(p-q)^{2}}{pq}}\quad {\text{with}}\quad p,q\in \mathbb {N} ^{*}}$

A W(N)-minimal model with central charge ${\displaystyle c_{k+N,k+N+1}}$ may be constructed as a coset of Wess-Zumino-Witten models ${\displaystyle {\frac {SU(N)_{k}\times SU(N)_{1}}{SU(N)_{k+1}}}}$. ^[11]

For example, the two-dimensional critical three-state Potts model has central charge ${\displaystyle c_{5,6}^{(2)}=c_{4,5}^{(3)}={\frac {4}{5}}}$. Spin observables of the model may be described in terms of the D-series non-diagonal Virasoro minimal model with ${\displaystyle (p,q)=(5,6)}$, or in terms of the diagonal W(3)-minimal model with ${\displaystyle (p,q)=(4,5)}$.

Conformal Toda theory

Conformal Toda theory is a generalization of Liouville theory that is based on a W-algebra. Given a simple Lie algebra ${\displaystyle {\mathfrak {g}}}$, the Lagrangian is a functional of a field ${\displaystyle \phi }$ which belongs to the root space of ${\displaystyle {\mathfrak {g}}}$, with one interaction term for each simple root:

${\displaystyle L[\phi ]={\frac {1}{2\pi }}(\partial \phi ,{\bar {\partial }}\phi )+\mu \sum _{e\in \{{\text{simple roots of }}{\mathfrak {g}}\}}\exp \left(b(e,\phi )\right)}$

This depends on the cosmological constant ${\displaystyle \mu }$, which plays no meaningful role, and on the parameter ${\displaystyle b}$, which is related to the central charge. The resulting field theory is a conformal field theory, whose chiral symmetry algebra is a W-algebra constructed from ${\displaystyle {\mathfrak {g}}}$ by Drinfeld-Sokolov reduction. For the preservation of conformal symmetry in the quantum theory, it is crucial that there are no more interaction terms than components of the vector ${\displaystyle \phi }$. ^[4]

The methods that lead to the solution of Liouville theory may be applied to W(N)-conformal Toda theory, but they only lead to the analytic determination of a particular class of three-point structure constants, ^[10] and W(N)-conformal Toda theory with ${\displaystyle N\geq 3}$ has not been solved.

Logarithmic conformal field theory

At central charge ${\displaystyle c=c_{1,q}^{(2)}}$, the Virasoro algebra can be extended by a triplet of generators of dimension ${\displaystyle 2q-1}$, thus forming a W-algebra with the set of dimensions ${\displaystyle H=\{2,2q-1,2q-1,2q-1\}}$. Then it is possible to build a rational conformal field theory based on this W-algebra, which is logarithmic. ^[12] The simplest case is obtained for ${\displaystyle q=2}$, has central charge ${\displaystyle c=-2}$, and has been particularly well studied, including in the presence of a boundary. ^[13]

Related concepts

Finite W-algebras

Finite W-algebras are certain associative algebras associated to nilpotent elements of semisimple Lie algebras. ^[14]

The original definition, provided by Alexander Premet, starts with a pair ${\displaystyle ({\mathfrak {g}},e)}$ consisting of a reductive Lie algebra ${\displaystyle {\mathfrak {g}}}$ over the complex numbers and a nilpotent element e. By the Jacobson-Morozov theorem, e is part of a sl₂ triple (e, h, f). The eigenspace decomposition of ad(h) induces a ${\displaystyle \mathbb {Z} }$-grading on ${\displaystyle {\mathfrak {g}}}$:

${\displaystyle {\mathfrak {g}}=\bigoplus {\mathfrak {g}}(i).}$

Define a character ${\displaystyle \chi }$ (i.e. a homomorphism from ${\displaystyle {\mathfrak {g}}}$ to the trivial 1-dimensional Lie algebra) by the rule ${\displaystyle \chi (x)=\kappa (e,x)}$, where ${\displaystyle \kappa }$ denotes the Killing form. This induces a non-degenerate anti-symmetric bilinear form on the −1 graded piece by the rule:

${\displaystyle \omega _{\chi }(x,y)=\chi ([x,y]).}$

After choosing any Lagrangian subspace ${\displaystyle l}$, we may define the following nilpotent subalgebra which acts on the universal enveloping algebra by the adjoint action.

${\displaystyle {\mathfrak {m}}=l+\bigoplus _{i\leq -2}{\mathfrak {g}}(i).}$

The left ideal ${\displaystyle I}$ of the universal enveloping algebra ${\displaystyle U({\mathfrak {g}})}$ generated by ${\displaystyle \{x-\chi (x):x\in {\mathfrak {m}}\}}$ is invariant under this action. It follows from a short calculation that the invariants in ${\displaystyle U({\mathfrak {g}})/I}$ under ad${\displaystyle ({\mathfrak {m}})}$ inherit the associative algebra structure from ${\displaystyle U({\mathfrak {g}})}$. The invariant subspace ${\displaystyle (U({\mathfrak {g}})/I)^{{\text{ad}}({\mathfrak {m}})}}$ is called the finite W-algebra constructed from ${\displaystyle ({\mathfrak {g}},e)}$, and is usually denoted ${\displaystyle U({\mathfrak {g}},e)}$.

References

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2. Watts, Gerard M. T. (1997). "W-algebras and their representations" (PDF). In Horváth, Zalán; Palla, László (eds.). Conformal field theories and integrable models (Budapest, 1996). Lecture Notes in Phys. Vol. 498. Berlin, New York: Springer-Verlag. pp. 55–84. doi:10.1007/BFb0105278. ISBN   978-3-540-63618-2. MR   1636798. S2CID   117999633.
3. de Boer, J.; Fehér, L.; Honecker, A. (1994). "A class of -algebras with infinitely generated classical limit". Nuclear Physics B. Elsevier BV. 420 (1–2): 409–445. arXiv: hep-th/9312049 . Bibcode:1994NuPhB.420..409D. doi:10.1016/0550-3213(94)90388-3. ISSN   0550-3213. S2CID   11747034.
4. Litvinov, Alexey; Spodyneiko, Lev (2016). "On W algebras commuting with a set of screenings". Journal of High Energy Physics. 2016 (11): 138. arXiv: 1609.06271 . Bibcode:2016JHEP...11..138L. doi:10.1007/jhep11(2016)138. ISSN   1029-8479. S2CID   29261029.
5. Creutzig, Thomas; Hikida, Yasuaki; Rønne, Peter B. (2016). "Correspondences between WZNW models and CFTs with W-algebra symmetry". Journal of High Energy Physics. 2016 (2): 48. arXiv: 1509.07516 . Bibcode:2016JHEP...02..048C. doi:10.1007/jhep02(2016)048. ISSN   1029-8479. S2CID   44722579.
6. Bouwknegt, Peter; Schoutens, Kareljan (1993). "W symmetry in conformal field theory". Physics Reports. 223 (4): 183–276. arXiv: hep-th/9210010 . Bibcode:1993PhR...223..183B. doi:10.1016/0370-1573(93)90111-P. ISSN   0370-1573. MR   1208246. S2CID   118959569.
7. De Vos, Koos; van Driel, Peter (1996). "The Kazhdan–Lusztig conjecture for W algebras". Journal of Mathematical Physics. AIP Publishing. 37 (7): 3587–3610. arXiv: hep-th/9508020 . Bibcode:1996JMP....37.3587D. doi:10.1063/1.531584. ISSN   0022-2488. S2CID   119348884.
8. Watts, G. M. T. (1995). "Fusion in the W3 algebra". Communications in Mathematical Physics. 171 (1): 87–98. arXiv: hep-th/9403163 . doi:10.1007/bf02103771. ISSN   0010-3616. S2CID   86758219.
9. Fateev, Vladimir; Ribault, Sylvain (2010). "Conformal Toda theory with a boundary". Journal of High Energy Physics. 2010 (12): 089. arXiv: 1007.1293 . Bibcode:2010JHEP...12..089F. doi:10.1007/jhep12(2010)089. ISSN   1029-8479. S2CID   17631088.
10. Fateev, V.A; Litvinov, A.V (2007-11-05). "Correlation functions in conformal Toda field theory I". Journal of High Energy Physics. 2007 (11): 002. arXiv: 0709.3806 . Bibcode:2007JHEP...11..002F. doi:10.1088/1126-6708/2007/11/002. ISSN   1029-8479. S2CID   8189544.
11. Chang, Chi-Ming; Yin, Xi (2012). "Correlators in W N minimal model revisited". Journal of High Energy Physics. 2012 (10). arXiv: 1112.5459 . doi:10.1007/jhep10(2012)050. ISSN   1029-8479. S2CID   119114132.
12. Gaberdiel, Matthias R.; Kausch, Horst G. (1996). "A rational logarithmic conformal field theory". Physics Letters B. Elsevier BV. 386 (1–4): 131–137. arXiv: hep-th/9606050 . Bibcode:1996PhLB..386..131G. doi:10.1016/0370-2693(96)00949-5. ISSN   0370-2693. S2CID   13939686.
13. Gaberdiel, Matthias R; Runkel, Ingo (2006-11-08). "The logarithmic triplet theory with boundary". Journal of Physics A: Mathematical and General. 39 (47): 14745–14779. arXiv: hep-th/0608184 . Bibcode:2006JPhA...3914745G. doi:10.1088/0305-4470/39/47/016. ISSN   0305-4470. S2CID   10719319.
14. Wang, Weiqiang (2011). "Nilpotent orbits and finite W-algebras". In Neher, Erhard; Savage, Alistair; Wang, Weiqiang (eds.). Geometric representation theory and extended affine Lie algebras. Fields Institute Communications Series. Vol. 59. Providence RI. pp. 71–105. arXiv: 0912.0689 . Bibcode:2009arXiv0912.0689W. ISBN   978-082185237-8. MR   2777648.

Further reading

• de Boer, Jan; Tjin, Tjark (1993), "Quantization and representation theory of finite W algebras", Communications in Mathematical Physics, 158 (3): 485–516, arXiv: hep-th/9211109 , Bibcode:1993CMaPh.158..485D, doi:10.1007/bf02096800, ISSN   0010-3616, MR   1255424, S2CID   204933347
• Bouwknegt, P.; Schoutens, K., eds. (1995), W-symmetry, Advanced Series in Mathematical Physics, vol. 22, River Edge, New Jersey: World Scientific Publishing Co., doi:10.1142/2354, ISBN   978-981021762-4, MR   1338864
• Brown, Jonathan, Finite W-algebras of Classical Type (PDF)
• Dickey, L. A. (1997), "Lectures on classical W-algebras", Acta Applicandae Mathematicae, 47 (3): 243–321, doi:10.1023/A:1017903416906, ISSN   0167-8019, S2CID   118573600
• Gan, Wee Liang; Ginzburg, Victor (2002), "Quantization of Slodowy slices", International Mathematics Research Notices, 2002 (5): 243–255, arXiv: math/0105225 , doi: 10.1155/S107379280210609X , ISSN   1073-7928, MR   1876934, S2CID   13895488
• Losev, Ivan (2010), "Quantized symplectic actions and W-algebras", Journal of the American Mathematical Society , 23 (1): 35–59, arXiv: 0707.3108 , Bibcode:2010JAMS...23...35L, doi:10.1090/S0894-0347-09-00648-1, ISSN   0894-0347, MR   2552248, S2CID   16211165
• Pope, C.N. (1991), Lectures on W algebras and W gravity, Lectures given at the Trieste Summer School in High-Energy Physics, August 1991, arXiv: hep-th/9112076 , Bibcode:1991hep.th...12076P