Abstract
A variation of the Zamolodchikov–Faddeev algebra over a finitedimensional Hilbert space \({\mathcal {H}}\) and an involutive unitary RMatrix S is studied. This algebra carries a natural vacuum state, and the corresponding Fock representation spaces \({\mathcal {F}}_S({\mathcal {H}})\) are shown to satisfy \({\mathcal {F}}_{S\boxplus R}({{\mathcal {H}}}\oplus {{\mathcal {K}}}) \cong {\mathcal {F}}_S({{\mathcal {H}}})\otimes {\mathcal {F}}_R({{\mathcal {K}}})\), where \(S\boxplus R\) is the boxsum of S (on \({{\mathcal {H}}}\otimes {{\mathcal {H}}}\)) and R (on \({{\mathcal {K}}}\otimes {{\mathcal {K}}}\)). This analysis generalises the wellknown structure of Bose/Fermi Fock spaces and a recent result of Pennig. These representations are motivated from quantum field theory (shortdistance scaling limits of integrable models).
Similar content being viewed by others
1 Introduction
The Zamolodchikov–Faddeev algebras were introduced by the Zamolodchikov and Faddeev as a tool to describe integrable quantum field theories in which the full Smatrix factorises into products of 2particle Smatrices [8, 25]. These algebras (called ZF algebras for short) are generated by “creation” and “annihilation” operators obeying quadratic exchange relations given by the 2particle Smatrix. ZF algebras generalise the familiar CCR and CAR algebras [3] and are closely related to Wick algebras that allow normal ordering [11]. Hilbert space representations of ZF algebras are of central importance in integrable quantum field theory (see, for example, [1, 5, 14, 18, 24] for a few sample publications from a very large body of literature) as well as in other fields such as qdeformations [20, 22] or anyonic statistics [15].
The central datum defining the relations in a ZF algebra is a solution of the Yang–Baxter equation. In the QFT context, this solution plays the role of elastic twoparticle scattering matrix and depends on a spectral parameter (rapidity), i.e. it is a matrixvalued function \({{\mathbb {R}}}\ni \theta \mapsto \mathbf{S} (\theta )\in \text {End}({{\mathcal {H}}}\otimes {\mathcal {H}})\), where \({\mathcal {H}}\) is a finitedimensional Hilbert space.
The present work has its background in an ongoing research project about shortdistance scaling limits of integrable quantum field theories on twodimensional Minkowski space [23]. At finite scale, the QFTs that we have in mind are specified in an inverse scattering approach in terms of a mass parameter \(m>0\) and a Fock (vacuum) representation of the ZF algebra given by a twoparticle Smatrix \({{\mathbb {R}}}\ni \theta \mapsto \mathbf{S} (\theta )\in \text {End}({{\mathcal {H}}}\otimes {\mathcal {H}})\), subject to the usual constraints of unitarity, Poincaré invariance, Hermitian analyticity, and crossing symmetry. Under suitable regularity assumptions, a quantum field theory which has \(\mathbf{S} \) as its twoparticle Smatrix exists and can be constructed in the framework of algebraic quantum field theory [10] from m and \(\mathbf{S} \) alone, without reference to a Lagrangian (see [14] for a review of this construction).
It is then an interesting question to study the conformal chiral shortdistance scaling limit of these theories, generalising previous work on scalar (meaning \({{{\mathcal {H}}}}={\mathbb {C}}\)) models [2]. In our inverse scattering approach, field operators that are localised in Rindler wedges can be constructed explicitly in terms of the Fock representation of the ZF algebra, but the physical fields are characterised only indirectly. Hence, it is not clear for which \(\mathbf{S} \) the scaling limit exists as a local QFT or what its properties are (although this is investigated in many specific models [9]).
It is known, however, that existence of the two limits \(S_\pm :=\lim _{\theta \rightarrow \pm \infty }{} \mathbf{S} (\theta )\) is a necessary condition for the existence of the scaling limit, and local chiral fields have to satisfy specific commutation relations with representations (of the symmetric or braid groups) derived from \(S_\pm \). Furthermore, the value \(S_0:=\mathbf{S} (0)\) of the Smatrix at zero rapidity transfer determines the (anti)commutation relations between the chiral theories on the two opposite lightrays. Thus the three \(\theta \)independent unitary solutions \(S_0,S_+,S_\) of the Yang–Baxter equation (we will refer to unitary solutions to the Yang–Baxter equation as “Rmatrices” in this article) derived from \(\mathbf{S} \) govern essential properties of the scaling limit theories.
This motivates a closer study of representations of ZF algebras built from Rmatrices, which is the subject of this article. The properties of twoparticle Smatrices imply that \(S_0\) is involutive (meaning \(S_0^2=1\)) and \(S_+^*=S_\). In many examples (such as diagonal Smatrices or the Smatrix of the O(N) sigma models), the limits \(S_\pm \) are involutive as well. Although our arguments in this article are completely independent of QFT models, we take this physical background into account and mostly consider ZF algebras built from involutive Rmatrices. This enables us to use and apply recently established tools and results about the mathematical structure of the space of all involutive Rmatrices [16], denoted \({{\mathcal {R}}}_0({{\mathcal {H}}})\) for base space \({{\mathcal {H}}}\).
In Sect. 2, we define ZF algebras as abstract unital \({}^*\)algebras and their natural normalised vacuum functional \(\omega \). Section 3 is then devoted to an analysis of Fock representations. If \(\omega \) is positive as a functional (hence a state), these Fock representations coincide with the representations given by the general Gelfand–Naimark–Segal (GNS) construction applied to the ZF algebra w.r.t. \(\omega \). However, in general it is not initially clear that \(\omega \) is positive, and an independent construction has to be given. We do this by adapting a concrete representation known from quantum field theory to our setting and verify the GNS property afterwards (Theorem 3.4). Given the ZF algebra based on an involutive Rmatrix \(S\in {{\mathcal {R}}}_0({{\mathcal {H}}})\), this provides us with an Ssymmetric Fock representation space \({{\mathcal {F}}}_S({{\mathcal {H}}})\). For special choices of S, this coincides with the Bose or Fermi Fock space over \({{\mathcal {H}}}\).
In Sects. 4 and 5, we study the dependence of \({{\mathcal {F}}}_S({{\mathcal {H}}})\) on S. Adopting the boxsum operation \(\boxplus \) on \(\bigcup _{{\mathcal {H}}}{{\mathcal {R}}}_0({{\mathcal {H}}})\) from [16] (which yields \(R\boxplus S\in {{\mathcal {R}}}_0({{\mathcal {H}}}\oplus {{\mathcal {K}}})\) for \(R\in {{\mathcal {R}}}_0({{\mathcal {H}}})\), \(S\in {{\mathcal {R}}}_0({{\mathcal {K}}})\)), we prove
in Theorem 5.3 as our main result. It is interesting to note that for the case that all resulting Fock spaces are finitedimensional (which requires R, S to have “Fermionic” behaviour), such an isomorphism was recently proven by Pennig [21] with quite different methods as part of his classification of polynomial exponential functors on the category of finitedimensional Hilbert spaces. As required for applications in quantum field theory, our result holds for infinitedimensional Fock spaces and does not only give an isomorphism of Hilbert spaces, but also an isomorphism of representations of ZF algebras.
Isomorphism (1.1) is of particular interest because up to a natural notion of equivalence, every involutive Rmatrix can be written as an iterated boxsum of finitely many very simple \((\pm 1)\)Rmatrices [16]. In the QFT context, these correspond to free field theories, and the resulting decomposition of the Fock spaces and representations of ZF algebras could turn out to be a tool to investigate whether the scaling limit is isomorphic to a free field theory. As a first step in this direction, we investigate in Sect. 5 under which conditions we may identify our Fock representation with tensor products of simpler ones, providing examples and counterexamples.
Applications of our findings to the mentioned quantum field theoretic models and an analysis of their shortdistance scaling limits will appear in a future work.
2 An abstract ZF algebra
We begin by abstractly defining a variation of the wellknown Zamolodchikov–Faddeev algebra [8, 25]. Let \({\mathcal {L}}\) be a (separable) Hilbert space and S be a set of \(d^4\) (\(d\in {\mathbb {N}}\)) complex numbers whose elements are labelled by symbols \(S^{\alpha \beta }_{\delta \gamma }\) where \(\alpha , \beta ,\delta ,\gamma \in \{1, \ldots , d\}\). We then define the unital \(*\)algebra \({\mathcal {Z}}(S, {\mathcal {L}})\) as the algebra generated by the symbols \(1_{{\mathcal {Z}}(S, {\mathcal {L}})}, Z_{1}(f), Z_2(f), \ldots , Z_d(f)\) for all \(f\in {\mathcal {L}}\) which obey the following exchange relations:
where we understand that the repeated indices in an expression imply the sum over all possible values (Einstein summation convention).
We may view S as a linear map over the tensor square of a Hilbert space \({\mathcal {H}}\) of dimension d. Then the numbers \(S^{\alpha \beta }_{\delta \gamma }\) can be viewed as the matrix elements \(\langle e_{\alpha } \otimes e_{\beta }, S(e_{\delta } \otimes e_{\gamma })\rangle \), where \((e_{\alpha })_{\alpha =1}^{d_{{\mathcal {H}}}}\) is an orthonormal basis of \({\mathcal {H}}\).
A class of algebras related to ZF algebras, the socalled Wick algebras, are defined by omitting (2.2) from the definition. Their representations have been studied in [6, 11, 12].
At this stage it is not at all clear whether or not there exist Hilbert space representations of \({\mathcal {Z}}(S, {\mathcal {L}})\)—for example, in [11, p. 18] it is shown that for certain choices of S the corresponding Wick algebra admits no Hilbert space representations. As we will see, under certain assumptions on S a GNS representation of \({\mathcal {Z}}(S,{\mathcal {L}})\) can be constructed.
The notion of Wick ordering (sometimes also known as “normal” ordering) is a prolific and useful concept in the analysis of these algebras. To write an element \(X\in {\mathcal {Z}}(S, {\mathcal {L}})\) in Wick ordered form means to apply the governing relation (2.2) such that X becomes of the form
where \(\zeta _{\varvec{\eta }, \varvec{\xi }} \in {\mathbb {C}}\). The multiindex notation we have adopted here can be read as, for example,
where all \(f_{\eta _{n}} \in {\mathcal {L}}\) and \(\varvec{\eta } = N \in {\mathbb {N}}_0\) and in case \(\varvec{\eta } =0\), we take \(Z^*_{\varvec{\eta }}(f_{\varvec{\eta }}) = 1_{{\mathcal {Z}}(S, {\mathcal {L}})}\). We also remark that for the case of \(\varvec{\eta } = \varvec{\xi } = 0\) we have just a multiple of the identity in (2.3). Every element of \({\mathcal {Z}}(S,{\mathcal {L}})\) can be written in Wick ordered form. The Wick ordered form is typically not unique as we may exchange any two Z or \(Z^*\) elements in the expression using (2.1). However, the term with \(\varvec{\eta } = \varvec{\xi } =0\)is unique.
This discussion facilitates the definition of a linear functional over \({\mathcal {Z}}(S, {\mathcal {L}})\) and in particular proves it to be uniquely defined by the properties specified in the following definition.
Definition 2.1
We define a normalised linear functional \(\omega : {\mathcal {Z}}(S, {\mathcal {L}}) \rightarrow {\mathbb {C}}\) by the properties
 (i)$$\begin{aligned} \omega (1_{ {\mathcal {Z}}(S, {\mathcal {L}})}) = 1, \end{aligned}$$(2.4)
 (ii)$$\begin{aligned} \omega (Z^*_{\alpha }(f)\cdot X) =0, \end{aligned}$$(2.5)
 (iii)$$\begin{aligned} \omega (X\cdot Z_{\alpha }(f)) =0, \end{aligned}$$(2.6)
for all \(\alpha \in \{1,\ldots , d\}\), \(f\in {\mathcal {L}}\) any \(X \in {\mathcal {Z}}(S, {\mathcal {L}})\).
Defining a second functional as \(\lambda (X) := \overline{\omega (X^*)}\) and applying uniqueness, we see that \(\omega \) is Hermitian, but it is not necessarily positive.
Example 2.2
We consider here some simple examples of \({\mathcal {Z}}(S,{\mathcal {L}})\).
If we take first \(S^{ \beta \alpha }_{\delta \gamma } = \pm \delta ^{\alpha }_{\delta }\delta ^{\beta }_{\gamma }\), where \(\delta \) is the Kronecker delta, relations (2.1) and (2.2) now read (for \(f,g \in {\mathcal {L}}\))
Choosing an orthonormal basis \((e_{\alpha })_{\alpha =1}^d\) of \({\mathbb {C}}^d\), one realises that the elements \(a(\cdot )\) defined as \(a(e_{\alpha }\otimes f) := Z_{\alpha }(f) \) satisfy the governing relations of the CCR\(({\mathbb {C}}^d \otimes {\mathcal {L}})\) (\(+\)) and CAR\(({\mathbb {C}}^d \otimes {\mathcal {L}})\) (−) algebras [3, 7], respectively. We will note more on their representations in the next section. If we instead take \(S^{\alpha \beta }_{\delta \gamma } =  \delta ^{\alpha }_{\delta } \delta ^{\beta }_{\gamma }\), the governing relations become
This example is interesting in the context of Fock representations (which we will discuss in the next section), but for now we simply note that this example is also explored for the case of \({\mathcal {L}} = {\mathbb {C}}\) in [11, p. 48] in a Wick algebraic setting as a “degenerate case”.
3 Fock representations
We now consider (pre)Hilbert space representations of \({\mathcal {Z}}(S,{\mathcal {L}})\). To this end, we take the tensor product \(\tilde{{\mathcal {H}}} := {\mathcal {H}} \otimes {\mathcal {L}}\) (we reserve the notation of the tilde signifying the tensor product with \({\mathcal {L}}\)) of a Hilbert space \({\mathcal {H}}\) (of finite dimension \(d_{{\mathcal {H}}}\)) and the second internal space \({\mathcal {L}}\) for which we do not specify (or require) finite dimensionality. As mentioned previously, we may fix an orthonormal basis \((e_\alpha )_{\alpha =1}^{d_{{{\mathcal {H}}}}}\) of \({{{\mathcal {H}}}}\) and view the parameters \(S^{\alpha \beta }_{\delta \gamma }\) in (2.1,2.2) as the matrix elements \(S^{\alpha \beta }_{\delta \gamma } = \langle e_{\alpha }\otimes e_{\beta }, S(e_{\delta }\otimes e_{\gamma })\rangle \) of a linear map \(S:{{\mathcal {H}}}\otimes {{\mathcal {H}}}\rightarrow {{\mathcal {H}}}\otimes {{\mathcal {H}}}\).
As discussed in Introduction, construction in quantum field theory motivates us to consider the case that S solves the Yang–Baxter equation and is involutive. Note that S solving the Yang–Baxter equation implies that \({\mathcal {Z}}(S, {\mathcal {L}})\) is associative.
Definition 3.1
Let \({\mathcal {H}}\) be a Hilbert space. An involutive Rmatrix on \({\mathcal {H}}\) is a unitary, involutive map \(S\in {\mathcal {B}}({\mathcal {H}}\otimes {\mathcal {H}})\) that solves the Yang–Baxter equation. That is
We also denote by \({\mathcal {R}}_0({\mathcal {H}})\) the set of all involutive Rmatrices on \({\mathcal {H}}\).
We will mostly be interested in the case where \({\mathcal {H}}\) is finitedimensional (which we will always explicitly state), otherwise we always take \({\mathcal {H}}\) to be separable.
Before beginning the discussion of representations of \({\mathcal {Z}}(S,{\mathcal {L}})\), it is necessary to extend the definition of S to involve the space \({\mathcal {L}}\) and to do so we introduce the unitary operator \(U_n : \left( {\mathcal {H}} \otimes {\mathcal {L}}\right) ^{\otimes n} \rightarrow {\mathcal {H}}^{\otimes n} \otimes {\mathcal {L}}^{\otimes n}\) defined by
We can easily see that \(U_n\) is unitary from the above expression and it can be thought of as “disentangling” contributions from both Hilbert spaces, which induces an isomorphism between the domain and codomain of \(U_n\); hence, we will explicitly describe data acting only on \({\mathcal {H}}^{\otimes n} \otimes {\mathcal {L}}^{\otimes n}\) in this section. Employing the bounded linear operator \({\mathcal {B}}({\mathcal {L}}\otimes {\mathcal {L}}) \ni F:= F_{{\mathcal {L}}}\) (the tensor flip), we write
which one readily checks is still unitary, involutive and a solution to the Yang–Baxter equation. Though this is the explicit operator used in the construction, the interest is mostly in the contributions from S, and so we will avoid using \(S_F\) in further notation where possible.
We would like to consider the GNS representation of \({\mathcal {Z}}(S, {\mathcal {L}})\) with respect to the functional \(\omega \), but at this stage it is unclear whether \(\omega \) is positive. Instead, we will independently construct a representation of \({\mathcal {Z}}(S, {\mathcal {L}})\) and show it has the GNS property.
We choose an orthonormal basis \((e_{\alpha })_{\alpha =1}^{d_{{\mathcal {H}}}}\) of \({\mathcal {H}}\) and also make use of multiindex notation where we take \(e_{\varvec{\alpha }}\in {\mathcal {H}}^{\otimes n}\) to mean \(e_{\alpha _1} \otimes \cdots \otimes e_{\alpha _n}\).
Let \(S\in {\mathcal {R}}_0({\mathcal {H}})\), then we recall the structure of a Hilbert space representation of \({\mathcal {Z}}(S, {\mathcal {L}})\) as laid in a field theoretic setting in [17]. Denote by \(S_{k,n} := 1^{\otimes (k1)} \otimes S\otimes 1^{\otimes (nk1)}\) (where \(S(e_{\alpha }\otimes e_{\beta }) = S^{\gamma \delta }_{\alpha \beta } e_{\gamma }\otimes e_{\delta }\)) then we construct unitary operators on \({\mathcal {H}}^{\otimes n}\otimes {\mathcal {L}}^{\otimes n}\):
where \(\tau _i \in {\mathfrak {S}}_n\) (the symmetric group of n letters) is a transposition, swapping nearest neighbour i and \((i+1)\)th elements. It is straightforward to see that these operators generate a unitary representation of \({\mathfrak {S}}_n\) on \({\mathcal {H}}^{\otimes n}\otimes {\mathcal {L}}^{\otimes n}\), and then we can define an orthogonal projection [17] by taking their mean:
Define now the spaces
then the Ssymmetrised Fock space is given by
For (3.3) to be a unitary representation of \({\mathfrak {S}}_n\), involutivity of S is a crucial property. Dropping involutivity, unitary Rmatrices only give representations of the Braid groups. The concept of an Ssymmetric Fock space can be generalised to noninvolutive S [19], but it won’t play a role in the current work.
On this space, we have a vacuum vector \(\Omega _S = 1\oplus 0 \oplus ...\), and a dense subspace \({\mathcal {F}}^0_{S}(\tilde{{\mathcal {H}}})\) (consisting of vectors of “finite particle” number, meaning they are terminating direct sums of elements in increasing tensor powers). There is a natural unitary U from \({\mathcal {F}}_S(\tilde{{\mathcal {H}}})\) to the “disentangled Fock space” \(\bigoplus _n P_n^S({\mathcal {H}}^{\otimes n}\otimes {\mathcal {L}}^{\otimes n})=: \bigoplus _n {\mathcal {D}}_n(\tilde{{\mathcal {H}}})\), namely \(U=\bigoplus _n U_n\) is the second quantisation of the unitaries \(U_n\) (3.2). We may therefore treat operators on \({\mathcal {F}}_S(\tilde{{\mathcal {H}}})\) and \(U{\mathcal {F}}_S(\tilde{{\mathcal {H}}})\) on the same footing. To discuss the Fock representation of \({\mathcal {Z}}(S, {\mathcal {L}})\), it is more convenient to work on the latter space, and we define
for \(v_n\in {\mathcal {H}}^{\otimes n}, f_n \in {\mathcal {L}}^{\otimes n}, g\in {\mathcal {L}}.\)
Remark 3.2
We can write the explicit action of \(z_S\) in terms of the scalar product on \(\tilde{{\mathcal {H}}}_n\) by
for \(w_{n1}\otimes h_{n1} \in {\mathcal {H}}^{\otimes (n1)}\otimes {\mathcal {L}}^{\otimes (n1)}\). These operators then restrict to the symmetrised spaces \({\mathcal {D}}_n(\tilde{{\mathcal {H}}})\). In braket notation, (3.5a) simply reads
We have defined \(z^*_S, z_S\) with basis vectors of \({\mathcal {H}}\) as arguments; however, we can extend the definition to operators \(z_S^*(\psi )\), \(\psi \in \tilde{{\mathcal {H}}}\) by linearity in their arguments (care to be taken when doing the same to \(z_S\) as it is antilinear in its argument).
For ease of notation, we will use the shorthand \(z_S(e_{\alpha } \otimes g) = z_{S,\alpha }(g)\), and the polynomial algebra generated by all \(z_{S, \alpha }(f), z_{S, \beta }^*(g), 1_{\tilde{{\mathcal {H}}}}\) we will denote by \({\mathcal {P}}_S\).
Proposition 3.3
The vacuum vector \(\Omega _S\) is cyclic for the algebra \({\mathcal {P}}_S\), that is, \({\mathcal {P}}_S\Omega _S \subset U {\mathcal {F}}_S(\tilde{{\mathcal {H}}})\) is dense.
Proof
Let \(\psi \in {\mathcal {F}}_S(\tilde{{\mathcal {H}}})\) such that \(\psi \) is orthogonal to \({\mathcal {P}}_S\Omega \). For any \(n \in {\mathbb {N}}_0\), and vectors \(f_1, \ldots , f_n \in {\mathcal {L}}\), \(\alpha _1,\ldots , \alpha _n \in \{1, \ldots , d_{{\mathcal {H}}}\}\) we then have
where we have used that the projection \(P_n^S\) is selfadjoint and leaves the symmetrised vector \(\psi \) invariant. Since vectors of the form \(e_{\alpha _1} \otimes \cdots \otimes e_{\alpha _n} \otimes f_1 \otimes \cdots \otimes f_n\) form a total set in \({\mathcal {H}}^{\otimes n}\otimes {\mathcal {L}}^{\otimes n}\), we conclude that \(\psi =0\). Thus \(\Omega _S\) is cyclic for \({\mathcal {P}}_S\). \(\square \)
Before moving to the next result, we note specific elements of \({\mathfrak {S}}_n\) as they will play an important role in the following proof—define \(\sigma _n := \tau _{n1} \tau _{n2} ... \tau _1 \in {\mathfrak {S}}_n\) which acts by taking the first element and moving it to the nth position.
Theorem 3.4
Let \({\mathcal {H}}\) be a finitedimensional Hilbert space and \(S \in {\mathcal {R}}_0({\mathcal {H}})\). Then the map \(\pi _S: {\mathcal {Z}}(S, {\mathcal {L}}) \rightarrow {\mathcal {P}}_S\) given by
extends to a unital \(*\)representation of \({\mathcal {Z}}(S, {\mathcal {L}})\) on \({\mathcal {F}}^0_S(\tilde{{\mathcal {H}}})\) with cyclic vector \(\Omega _S\) and
Proof
We show first that the operators \(z_{S, \alpha }(f), z^*_{S,\alpha }(f)\) satisfy (2.1) and (2.2) for all \(f \in {\mathcal {L}}, \alpha \in \{1,\ldots , d_{{\mathcal {H}}}\}\). Let \(v_n \otimes h_n \in {\mathcal {D}}_n(\tilde{{\mathcal {H}}})\), \(f, g\in {\mathcal {L}}\) then taking into account \(P_{n+2}^S = P_{n+2}^S S_{1, n+1} \otimes F_1\)
Given that n and \(v_n\otimes h_n\) were arbitrary, we read off
as operators on \({\mathcal {F}}^0_S(\tilde{{\mathcal {H}}})\). Taking adjoints of both sides and applying both the unitarity and involutivity of S, we arrive at equation (2.1).
For showing (2.2), we first compute the action of the first term righthand side on some \(v_n\otimes h_n \in {\mathcal {D}}_n(\tilde{{\mathcal {H}}})\). It is enough to do so on vectors of the form \(v_n = e_i\otimes v_{n1}\), \(h_n = a \otimes h_{n1}\)\((a\in {\mathcal {L}}, v_{n1}\otimes h_{n1} \in {\mathcal {D}}_{n1}(\tilde{{\mathcal {H}}}))\) as they form a total set in \({\mathcal {H}}^{\otimes n}\) and \({\mathcal {L}}^{\otimes n}\), respectively. We have:
Since \(v_{n1}\) and \(h_{n1}\) are correctly symmetrised, the action of the projection \(P_n^S\) in the final line simplifies. Namely, we need only sum over the permutations that shift the \(e_{\gamma }\) and g terms such that they appear in each tensor slot [13]; \(P_n^S = \frac{1}{n} \sum _{k=1}^n D_n^S(\sigma _k)\cdot 1\otimes P_{n1}^S\). The above now reads
Recall that the lefthand side also depends on \(e_i\) and a via the definitions \(v_n = e_i\otimes v_{n1}\), \(h_n = a \otimes h_{n1}\). To compute the lefthand side of (2.2), we now consider its scalar product with a \(w_n\otimes b_n := e_j \otimes w_{n1} \otimes c\otimes b_{n1} \in {\mathcal {D}}_n(\tilde{{\mathcal {H}}})\) in the scalar product:
Since \(v_n\) and \(h_n\) are correctly symmetrised, the projection \(P_{n+1}^S\) again simplifies as before. Noting further that \(\sigma _1 = 1,\) this gives:
To shift the index of the sum \(\sum _{k=2}^{n+1} D_{n+1}^S(\sigma _k)\), we note that it sums over the permutations shifting the \(e_{\beta }\) term through each tensor slot with the first term being the permutation given by just \(S_{1,n+1} \otimes F_{1} = D_{n+1}^S(\tau _1)\). If we extract this term from the sum, we can read the remaining terms as taking the second tensor slot and permuting through the remaining n slots with the first slot being untouched [13]. Concretely, this means that we can write this as
which we use and continue in the calculation:
Since all elements involved were arbitrary, we now read off what we have computed by comparing the righthand slot of the scalar product:
We can now read that (up to the contraction term) we have equality between (3.9) and (3.10), and thus, (2.2) is satisfied so \(\pi _S\) is indeed a representation of \({\mathcal {Z}}(S,{\mathcal {L}})\) on \(U{\mathcal {F}}_S^0(\tilde{{\mathcal {H}}})\).
Moreover, \(\Omega _S\) is cyclic for this representation by Proposition 3.3, and then, the GNS property follows once we realise that the functional defined by the righthand side of (3.8) satisfies the properties of \(\omega \) as outlined in Definition 2.1 since \(\Omega _S\) is a normalised vector and \(z_S\) annihilates it. \(\square \)
Remark 3.5
It is now apparent that \(\omega \) is positive (for \(S \in {\mathcal {R}}_0({\mathcal {H}})\)). For any \(X\in {\mathcal {Z}}(S, {\mathcal {L}})\):
Revisiting the examples outlined in the previous section, we see that for \(S^{\alpha \beta }_{\delta \gamma } = \pm \delta ^{\alpha }_{\gamma }\delta ^{\beta }_{\delta }\) we arrive at the totally symmetric (\(+\)) or totally antisymmetric (−) Fock space over \(\tilde{{\mathcal {H}}}\), usually known as the Bosonic and Fermionic Fock spaces, respectively.
The case of \(S^{\alpha \beta }_{\delta \gamma } = \delta ^{\alpha }_{\delta }\delta ^{\beta }_{\gamma }\) (\(S=1\)) results in a very small space for \({\mathcal {L}} = {\mathbb {C}}\): For this particular choice of S, the projection simplifies greatly to
where sgn\((\pi )\) is the sign of the permutation \(\pi \). There then only exists a zeroparticle space (multiples of the vacuum) and the single particle space \(\tilde{{\mathcal {H}}}\):
The other extreme is given by \(S = 1\) and \({\mathcal {L}} = {\mathbb {C}}\), which generates the full unsymmetrised (or “Boltzmann”) Fock space
In general, \({\mathcal {F}}_S({\mathcal {H}})\) “interpolates” between these two extreme cases.
4 Operations on Rmatrices and equivalences
In this work, we aim to generalise the following notion (sometimes referred to as an “exponential relation”, see, for example, [4] and references therein): Let \({\mathcal {H}}, {\mathcal {K}}\) be Hilbert spaces, and denote by \({\mathcal {F}}_{\pm }({\mathcal {H}})\) the Bosonic/Fermionic Fock space over \({\mathcal {H}}\). To keep touch with our earlier constructions, this corresponds to the Fock representation of the algebra \({\mathcal {Z}}(\pm F_{{\mathcal {H}}}, {\mathbb {C}})\), where \(F_{{\mathcal {H}}}\) is the tensor flip on \({\mathcal {H}}^{\otimes 2}\) (we simplify notation here using ± as a subscript to mean \(S = \pm F_{{\mathcal {H}}}\) to remain familiar with notation existing in the literature). Then it is well known that there exists a natural isomorphism
This isomorphism does not only hold as a Hilbert space isomorphism (which is trivial for the case of infinitedimensional separable Hilbert spaces), but also as an isomorphism of representations of the CCR/CAR algebras.
In the following, we will explore to which extent (4.1) generalises to our setting of Ssymmetric Fock spaces. As a prerequisite for doing so, we need to compare Rmatrices on tensor products and direct sums of Hilbert spaces. The relevant notions are recalled below.
Definition 4.1
[16] Let \({\mathcal {H}}, {\mathcal {K}}\) be Hilbert spaces, and \(S\in {\mathcal {R}}_0({\mathcal {H}}), R\in {\mathcal {R}}_0({\mathcal {K}})\). Then we define
 (i)
\(S\boxplus R : ({\mathcal {H}} \oplus {\mathcal {K}}) \otimes ({\mathcal {H}} \oplus {\mathcal {K}}) \rightarrow ({\mathcal {H}} \oplus {\mathcal {K}}) \otimes ({\mathcal {H}} \oplus {\mathcal {K}}) \) as
$$\begin{aligned}&S\boxplus R := S \oplus R \oplus F, \quad \text {on}\\&({\mathcal {H}} \oplus {\mathcal {K}}) \otimes ({\mathcal {H}} \oplus {\mathcal {K}}) = ({\mathcal {H}} \otimes {\mathcal {H}} ) \oplus ({\mathcal {K}} \otimes {\mathcal {K}}) \oplus ({\mathcal {H}} \otimes {\mathcal {K}}) \oplus ({\mathcal {K}} \otimes {\mathcal {H}}). \end{aligned}$$  (ii)
\(S\boxtimes R : {\mathcal {H}}\otimes {\mathcal {K}} \otimes {\mathcal {H}}\otimes {\mathcal {K}} \rightarrow {\mathcal {H}}\otimes {\mathcal {K}}\otimes {\mathcal {H}}\otimes {\mathcal {K}} \) as
$$\begin{aligned} S\boxtimes R = F_2(S\otimes R)F_2 \end{aligned}$$where \(F_2\) exchanges the second and third tensor factors.
We use the terminology boxsum and boxproduct, respectively, for these operations.
These two operations preserve unitarity, involutivity and if S, R are solutions to the Yang–Baxter equation, then \(S\boxplus R, S\boxtimes R\) are also solutions, and hence, we have that \(S\boxplus R \in {\mathcal {R}}_0({\mathcal {H}}\oplus {\mathcal {K}})\) and \(S\boxtimes R \in {\mathcal {R}}_0({\mathcal {H}} \otimes {\mathcal {K}})\) [16].
A generalisation of (4.1) that we will show in this work (for now setting \({\mathcal {L}} = {\mathbb {C}}\)) now reads as
where \(S\in {\mathcal {R}}_0({\mathcal {H}}), R\in {\mathcal {R}}_0({\mathcal {K}})\) for Hilbert spaces \({\mathcal {H}}, {\mathcal {K}}\). Setting \(S= F_{{\mathcal {H}}}, R= F_{{\mathcal {K}}}\), then \(S\boxplus R = F_{{\mathcal {H}} \oplus {\mathcal {K}}}\) and the above reads the same as (4.1) for the Bose case, so we at least realise immediately this is consistent with existing results.
Under the assumption that all resulting Fock spaces are finitedimensional, isomorphism (4.2) has recently been established by Pennig using exponential functors [21]. This assumption of finite dimensionality is satisfied, for example, by \(S=1\) or \(S=F_{{\mathcal {H}}}\), and more generally for all Rmatrices having only “Fermionic” Thoma parameters. For applications to quantum field theory, however, it is essential to have an infinitedimensional Hilbert space, and our setup and arguments in the following will be quite different from that of [21].
In addition, the analysis of equivalent functors in [21] also yielded an equivalence between functors when there is a natural equivalence between the Rmatrices associated with them. We may also wonder if it is possible to formulate such an isomorphism in our setting and to this end, we recall the notion of equivalent Rmatrices.
Definition 4.2
[16] Let \({\mathcal {H}}, {\mathcal {K}}\) be Hilbert spaces, \(S \in {\mathcal {R}}_0({\mathcal {H}}), R\in {\mathcal {R}}_0({\mathcal {K}})\), then they are said to be equivalent  denoted as \(S \sim R\)—if and only if, for each \(n \in {\mathbb {N}}\) the representations \(D_n^S\) and \(D_n^R\) are unitarily equivalent.
Let \(S\in {\mathcal {R}}_0({\mathcal {H}}), R\in {\mathcal {R}}_0({\mathcal {K}})\). If \(S \sim R\), this definition means that there exists a unitary intertwining operator \(Y^{S,R}_n : {\mathcal {H}}_n \rightarrow {\mathcal {K}}_n\) such that
In general, the form of \(Y_n^{S,R}\) is unknown, but we can provide a few examples [16] of when we may write down its action explicitely.
Type 1: There exists a unitary Q on \({\mathcal {H}}\) such that \((Q\otimes Q) S(Q^*\otimes Q^*) = R\). Then \(S\sim R\) and we may choose
$$\begin{aligned} Y_n^{S,R} = Q^{\otimes n}. \end{aligned}$$Type 2: There exists a unitary Q on \({\mathcal {H}}\) such that \([S, Q\otimes Q] =0\) and \((1\otimes Q)S(1\otimes Q^*) = R.\) Then \(S\sim R\) and we may choose
$$\begin{aligned} Y_n^{S,R} = 1\otimes Q \otimes \cdots \otimes Q^{n1}. \end{aligned}$$Type 3: Let \(F : {\mathcal {H}}^{\otimes 2}\rightarrow {\mathcal {H}}^{\otimes 2}\), \(F(x\otimes y) = y\otimes x, (x,y \in {\mathcal {H}})\) be the “flip” operator, such that \(FSF = R\). Then \(S\sim R\) and we may choose
$$\begin{aligned} Y_n^{S,R} = D_n^{FSF}(\iota _n)^{1}D_n^F(\iota _n) \end{aligned}$$where \(\iota _n\) is the total inversion permutation in n letters.
The significance of the equivalence relation \(\sim \) stems from the fact that every \(S\in {\mathcal {R}}_0({\mathcal {H}})\) is equivalent to a very simple Rmatrix, namely an Rmatrix of socalled normal form: It was shown in [16] that for any \(S\in {\mathcal {R}}_0({\mathcal {H}})\), there exists \(N\in {\mathbb {N}}\), dimension parameters \(d_1, \ldots , d_N \in {\mathbb {N}}\) with \(d_1+\cdots +d_N = d_{{\mathcal {H}}}\) and signs \(\varepsilon _1, \ldots , \varepsilon _N \in \{+1, 1\}\), such that
From this definition, we can read off that the tensor flip is a normal form, and also the identity (take \(N=1\) and \(\varepsilon _1 = +1\)), as examples. Considering now two equivalent Rmatrices \(S\sim R\), we may wonder whether we have an isomorphism
where this could simply be an isomorphism of Hilbert spaces, or even an isomorphism of representations of ZF algebras.
Since any Rmatrix S is equivalent to a normal form (4.4), the combination of the anticipated isomorphisms (4.5) and (4.2) would allow us to split \({\mathcal {F}}_S({\mathcal {H}})\) into a tensor product of Fock spaces of the simple form \({\mathcal {F}}_{\pm 1_{d_i^2}}({\mathcal {H}}_i)\).
As a preparatory step to the next section where we cement these ideas, we note the following results.
Lemma 4.3
Let \({\mathcal {H}}, {\mathcal {K}}\) be separable Hilbert spaces, and \(S\in {\mathcal {R}}_0({\mathcal {H}}), R\in {\mathcal {R}}_0({\mathcal {K}})\). Then the representation of the symmetric group, \(D_n^{S\boxtimes R},\) generated by \(S\boxtimes R\) is unitarily equivalent to \(D_n^S\otimes D_n^R\) for any \(n\in {\mathbb {N}}\).
Proof
We show the result for only the generating elements \(\tau _k\), of \({\mathfrak {S}}_n\). Let \((h_{\alpha })_{\alpha \in {\mathbb {N}}}\) and \((k_{\beta })_{\beta \in {\mathbb {N}}}\) be orthonormal bases of \({\mathcal {H}}\) and \({\mathcal {K}}\) respectively. Employing the operator \(U_n\), an element in the domain of \(D_n^{S\boxtimes R}\) is mapped to an element in the domain of \(D_n^S\otimes D_n^R\) and the action of the latter operator is given by
where the implicit sums converge in norm topology. Applying the linear operator \(U_n^*\) to the above gives the action of \(D_n^{S\boxtimes R}\) as stated. \(\square \)
Corollary 4.4
Let \({\mathcal {H}}_1, {\mathcal {H}}_2\), \({\mathcal {K}}_1, {\mathcal {K}}_2\) be Hilbert spaces, \(S_1 \in {\mathcal {R}}_0({\mathcal {H}}_1), R_1\in {\mathcal {R}}_0({\mathcal {K}}_1)\), \(S_2 \in {\mathcal {R}}_0({\mathcal {H}}_2), R_2 \in {\mathcal {R}}_0({\mathcal {K}}_2)\) such that \(S_1 \sim S_2\) and \(R_1 \sim R_2\) . Then an intertwiner for \(S_1\boxtimes R_1 \sim S_2\boxtimes R_2\), \(Y^{S_1\boxtimes R_1, S_2 \boxtimes R_2}\), is given by
with \(Y^{S_1, S_2}\), \(Y^{R_1, R_2}\) intertwiners between \(S_1, S_2\) and \(R_1, R_2\), respectively.
Proof
This is clear from the definition of \(U_n\) and Lemma 4.3. \(\square \)
We mention as an aside that an analogue of Corollary 4.4 also holds for boxsums \(S_1\boxplus R_1 \sim S_2\boxplus R_2\). As we will not need this here, we omit the details.
5 Isomorphisms between polynomial algebras and equivalences of representations
We now go on to discuss generalisations of (4.1), and in particular, we consider (4.2) with the addition of the Hilbert space \({\mathcal {L}}\) appearing in a tensor product with both \({\mathcal {H}}, {\mathcal {K}}\). For \(S\in {\mathcal {R}}_0({\mathcal {H}}), R\in {\mathcal {R}}_0({\mathcal {K}})\), define \(S\boxtimes F =: {\tilde{S}} \in {\mathcal {R}}_0(\tilde{{\mathcal {H}}})\), for F the tensor flip on \({\mathcal {L}}\otimes {\mathcal {L}}\), and similarly for R. As mentioned previously, the tilde appearing above Rmatrices always signifies a boxproduct with F, and above a Hilbert space always means a tensor product with the same space \({\mathcal {L}}\). With this notation, we will now aim to show the following:
On the lefthand side, the GNS representation is already described in Sect. 3, where we have a space symmetrised by the operator \(\tilde{S}\boxplus \tilde{R}\), but so far we have not considered representations of Zamolodchikov operators on \({\mathcal {F}}_{\tilde{S}}(\tilde{{\mathcal {H}}}) \otimes {\mathcal {F}}_{\tilde{R}}(\tilde{{\mathcal {K}}})\). We will first build data on this space—most notably the analogue of the creation/annihilation operators and vacuum vector. The exchange relations between the former and the cyclicity of the latter will be shown, before a GNStype argument will prove that they are in fact equivalent representations of the same algebra \({\mathcal {Z}}(S\boxplus R, {\mathcal {L}})\).
We begin with the algebra \({\mathcal {Z}}(S\boxplus R, {\mathcal {L}})\) as given in Sect. 1, with \(S\in {\mathcal {R}}_0({\mathcal {H}}), R\in {\mathcal {R}}_0({\mathcal {K}})\) and note a property regarding distributivity of the boxproduct over the boxsum. Generally, the distributivity property is only known up to equivalence, but in the specific cases considered in this work, we show that we in fact have equality.
Lemma 5.1
Let \({\mathcal {H}}, {\mathcal {K}}\) be finitedimensional Hilbert spaces, \(S\in {\mathcal {R}}_0({\mathcal {H}}), R\in {\mathcal {R}}_0({\mathcal {K}})\). Then
Proof
On the level of the spaces they act on, we first note that
where by \({\mathcal {D}}(S)\) we mean the domain of S.
To show they do indeed map vectors in their respective domains to the same vector, we consider each orthogonal component of their domains and discuss how each operator acts.
Firstly, the case of \(({\mathcal {H}} \otimes {\mathcal {L}})^{\otimes 2}\), the lefthand side of (5.2) first applies \(F_2\) and then acts as a flip in the \({\mathcal {L}}^{\otimes 2}\) parts, and as \(S\boxplus R\) on \({\mathcal {H}}^{\otimes 2}\) which by definition simply acts as just S, and finally applies a second \(F_2\). More simply put, it flips the contributions from \({\mathcal {L}}\) and acts as S on the contributions from \({\mathcal {H}}\). The same occurs on the righthand side of (5.2), where we see that it simply acts as only \(\tilde{S}\) by definition of the boxsum, which flips the contributions from \({\mathcal {L}}\) and acts as S on the contributions from \({\mathcal {H}}\).
Similarly, for the case of \(({\mathcal {K}} \otimes {\mathcal {L}})^{\otimes 2}\), the lefthand side of (5.2) flips on \({\mathcal {L}}\) and acts as R on \({\mathcal {K}}\). Identically, the righthand side of (5.2) acts just as \(\tilde{R}\) which again flips on \({\mathcal {L}}\) and acts as \({\mathcal {K}}\) and so we equality again.
The remaining cases to consider are \({\mathcal {H}} \otimes {\mathcal {L}} \otimes {\mathcal {K}} \otimes {\mathcal {L}}\) and \({\mathcal {K}} \otimes {\mathcal {L}} \otimes {\mathcal {H}}\otimes {\mathcal {L}}\). However, since we have a single contribution from both \({\mathcal {H}}\) and \({\mathcal {K}}\) appearing, each operator simply reduces to a combination of flips acting on the appropriate spaces and it is easy to realise that \(F_2(F_{{\mathcal {H}}\oplus {\mathcal {K}}} \otimes F)F_2 = F_{\tilde{{\mathcal {H}}}\otimes \tilde{{\mathcal {K}}}}\) and \(F_2(F_{{\mathcal {K}}\oplus {\mathcal {H}}} \otimes F)F_2 = F_{\tilde{{\mathcal {K}}}\otimes \tilde{{\mathcal {H}}}}\).
Both sides of (5.2) then act in the same way on each orthogonal part of their isomorphic domains, therefore they are equal. \(\square \)
The algebra of interest in this section, \({\mathcal {Z}}(S\boxplus R,{\mathcal {L}})\), is described by the operator \(\left( S\boxplus R\right) \boxtimes F\), but now Lemma 5.1 allows us to work instead with \(\tilde{S} \boxplus \tilde{R}\).
We consider the Fock space \({\mathcal {F}}_{\tilde{S} \boxplus \tilde{R}} (\tilde{{\mathcal {H}}} \oplus \tilde{{\mathcal {K}}})\) on which we have a vacuum vector \(\Omega _{\tilde{S} \boxplus \tilde{R}}\) and creation/annihilation operators \(z_{\tilde{S} \boxplus \tilde{R}}^*, z_{\tilde{S} \boxplus \tilde{R}}\). The latter obey exchange relations involving the operator \(\tilde{S} \boxplus \tilde{R},\) which we note here for convenience. We adopt the shorthand notation \(\tilde{{\mathcal {H}}} \ni f_{\alpha } := e_{\alpha } \otimes f\) for \(f\in {\mathcal {L}}\) and basis vectors \(e_{\alpha }\) of \({\mathcal {H}}\), and \(\tilde{{\mathcal {K}}} \ni g_{\xi } := k_{\xi } \otimes g\) for \(g\in {\mathcal {L}}\) and basis vectors \(k_{\xi }\) of \({\mathcal {K}}\). Then
These operators along with the identity \(1_{\tilde{{\mathcal {H}}}\oplus \tilde{{\mathcal {K}}}}\) generate the polynomial algebra \({\mathcal {P}}_{\tilde{S}\boxplus \tilde{R}}\) and form our natural Fock representation of the algebra \({\mathcal {Z}}(S \boxplus R, {\mathcal {L}})\).
We now consider a tensor product of Fock spaces
and on each Fock space, we have creation/annihilation operators \(z_{\tilde{S}}^*, z_{\tilde{S}}, z_{\tilde{R}}^*, z_{\tilde{R}}\) acting endomorphically on \({\mathcal {F}}_{\tilde{S}}^0(\tilde{{\mathcal {H}}}), {\mathcal {F}}_{\tilde{R}}^0(\tilde{{\mathcal {K}}})\) respectively; vacuum vectors \(\Omega _{\tilde{S}}, \Omega _{\tilde{R}}\) define similar data on \({\mathcal {F}}_{\tilde{S}}(\tilde{{\mathcal {H}}})\otimes {\mathcal {F}}_{\tilde{R}}(\tilde{{\mathcal {K}}}):\)
The polynomial algebra \({\mathcal {P}}_{\tilde{S}, \tilde{R}}\) is then defined as the algebra generated by the operators \(1_{\tilde{{\mathcal {H}}}}\otimes 1_{\tilde{{\mathcal {K}}}}, z^*_{\tilde{S}, \tilde{R}}, z_{\tilde{S}, \tilde{R}}\).
Lemma 5.2
The vacuum vector \(\Omega _{\tilde{S}, \tilde{R}}\) is cyclic for the polynomial algebra \({\mathcal {P}}_{\tilde{S}, \tilde{R}}\). That is, \({\mathcal {P}}_{\tilde{S}, \tilde{R}} \Omega _{\tilde{S}, \tilde{R}}\) is dense in \({\mathcal {F}}_{\tilde{S}}(\tilde{{\mathcal {H}}}) \otimes {\mathcal {F}}_{\tilde{R}}(\tilde{{\mathcal {K}}})\).
Proof
Let \(\psi \in {\mathcal {F}}_{\tilde{S}}(\tilde{{\mathcal {H}}})\otimes {\mathcal {F}}_{\tilde{R}}(\tilde{{\mathcal {K}}})\) be orthogonal to \({\mathcal {P}}_{\tilde{S}, \tilde{R}}\Omega _{\tilde{S}, \tilde{R}}\). Then for any \(i,j \in {\mathbb {N}}_0\) and vectors \(f_1, \ldots , f_i \in \tilde{{\mathcal {H}}}, g_1, \ldots , g_j \in \tilde{{\mathcal {K}}}\)
where \(\psi _{i,j}\) is the i, jth component of \(\psi \), each letter corresponding to each tensor slot in \({\mathcal {F}}_{\tilde{S}}(\tilde{{\mathcal {H}}}) \otimes {\mathcal {F}}_{\tilde{R}}(\tilde{{\mathcal {K}}})\) and we have used that the selfadjoint projection \(P_i^{\tilde{S}}\otimes P_j^{\tilde{R}}\) leaves the vector \(\psi \) invariant. By the definition of the tensor product, the vectors \( f_1\otimes \cdots \otimes f_i\otimes g_1\otimes \cdots \otimes g_j\) form a total set in \(\tilde{{\mathcal {H}}}^{\otimes i} \otimes \tilde{{\mathcal {K}}}^{\otimes j}\), and hence, we conclude that \(\psi =0\). \(\square \)
We are now ready to prove the claimed isomorphism of Fock spaces as representations of \({\mathcal {Z}}(S\boxplus R, {\mathcal {L}})\).
Theorem 5.3
Let \({\mathcal {H}}, {\mathcal {K}}\) be Hilbert spaces of finite dimensions \(d_{{\mathcal {H}}}, d_{{\mathcal {K}}}\), respectively, and \(\tilde{S}\in {\mathcal {R}}_0(\tilde{{\mathcal {H}}}), \tilde{R} \in {\mathcal {R}}_0(\tilde{{\mathcal {K}}})\), then:
 a)
The map \(\pi _{\tilde{S}, \tilde{R}}: {\mathcal {Z}}(S\boxplus R, {\mathcal {L}}) \rightarrow {\mathcal {P}}_{\tilde{S}, \tilde{R}}\)
$$\begin{aligned} \begin{aligned} \pi _{\tilde{S}, \tilde{R}}\left( 1_{{\mathcal {Z}}(S\boxplus R, {\mathcal {L}})}\right)&:= 1_{\tilde{{\mathcal {H}}}\otimes \tilde{{\mathcal {K}}}},\\ \pi _{\tilde{S}, \tilde{R}}(Z_{\alpha }(f))&:= {\left\{ \begin{array}{ll} z_{\tilde{S}, \tilde{R}}(f_{\alpha } \oplus 0), \ &{} \alpha \in \{1, \ldots , d_{{\mathcal {H}}}\}\\ z_{\tilde{S}, \tilde{R}}(0\oplus f_{\alpha d_{{\mathcal {H}}}}), \ &{} \alpha \in \{d_{{\mathcal {H}}} +1, \ldots , d_{{\mathcal {H}}}+d_{{\mathcal {K}}}\}\end{array}\right. } \end{aligned} \end{aligned}$$extends to a unital \(*\)representation of \({\mathcal {Z}}(S\boxplus R, {\mathcal {L}})\) on \({\mathcal {F}}^0_{\tilde{S}}(\tilde{{\mathcal {H}}}) \otimes {\mathcal {F}}^0_{\tilde{R}}(\tilde{{\mathcal {K}}})\) with cyclic vector \(\Omega _{\tilde{S}, \tilde{R}}\) and
$$\begin{aligned} \omega _{\tilde{S}, \tilde{R}}(X) = \langle \Omega _{\tilde{S}, \tilde{R}}, \pi _{\tilde{S}, \tilde{R}}(X)\Omega _{\tilde{S}, \tilde{R}}\rangle , \quad X\in {\mathcal {Z}}(S\boxplus R, {\mathcal {L}}). \end{aligned}$$(5.11)  b)
There exists a unitary \(V: {\mathcal {F}}_{\tilde{S}\boxplus \tilde{R}}(\tilde{{\mathcal {H}}} \oplus \tilde{{\mathcal {K}}}) \rightarrow {\mathcal {F}}_{\tilde{S}}(\tilde{{\mathcal {H}}}) \otimes {\mathcal {F}}_{\tilde{R}}(\tilde{{\mathcal {K}}})\) such that
$$\begin{aligned} V\Omega _{\tilde{S}\boxplus \tilde{R}} = \Omega _{\tilde{S}, \tilde{R}},\quad V\pi _{\tilde{S}\boxplus \tilde{R}}(X)V^* = \pi _{\tilde{S}, \tilde{R}}(X), \quad (X\in {\mathcal {Z}}(S\boxplus R, {\mathcal {L}})).\qquad \end{aligned}$$(5.12)
Proof

a)
We show first that the operators \(z_{\tilde{S}, \tilde{R}}^*, z_{\tilde{S}, \tilde{R}}\) satisfy the same relations as \(z_{\tilde{S}\boxplus \tilde{R}}^*, z_{\tilde{S}\boxplus \tilde{R}}\) as outlined in (5.3)–(5.8), firstly noting that
$$\begin{aligned} z_{\tilde{S}, \tilde{R}}(f_{\alpha }\oplus 0) = z_{\tilde{S},\alpha }(f)\otimes 1_{\tilde{{\mathcal {K}}}}, \quad z_{\tilde{S}, \tilde{R}}(0\oplus f_{\xi }) = 1_{\tilde{{\mathcal {K}}}}\otimes z_{\tilde{R}, \xi }(f), \quad (f\in {\mathcal {L}}), \end{aligned}$$and similarly for \(z^*_{\tilde{S}, \tilde{R}}\). Furthermore, the operators \(z_{\tilde{S}}^*, z_{\tilde{S}}\) and \(z_{\tilde{R}}^*, z_{\tilde{R}}\) satisfy exchange relations (2.1), (2.2) governed by S and R, respectively. Let \(f, g \in {\mathcal {L}}\) then
$$\begin{aligned} \begin{aligned} z_{\tilde{S}, \tilde{R}}(f_{\alpha }\oplus 0)z_{\tilde{S}, \tilde{R}}(g_{\beta }\oplus 0)&= z_{\tilde{S},\alpha }(f)z_{\tilde{S}, \beta }(g) \otimes 1_{\tilde{{\mathcal {K}}}} \\&= S^{\beta \alpha }_{\delta \gamma } z_{\tilde{S}, \gamma }(g)z_{\tilde{S},\delta }(f) \otimes 1_{\tilde{{\mathcal {K}}}} \\&= S^{\beta \alpha }_{\delta \gamma } z_{\tilde{S}, \tilde{R}}(g_{\gamma }\oplus 0)z_{\tilde{S}, \tilde{R}}(f_{\delta }\oplus 0), \end{aligned} \end{aligned}$$which gives (5.3). Relation (5.5) follows in an analogous way on the second tensor factor applying (2.1) for \(z_{\tilde{R}}\). Similarly
$$\begin{aligned} \begin{aligned} z_{\tilde{S}, \tilde{R}}(f_{\alpha }\oplus 0)z^*_{\tilde{S}, \tilde{R}}(g_{\beta }\oplus 0)&= z_{\tilde{S},\alpha }(f)z^*_{\tilde{S},\beta }(g) \otimes 1_{\tilde{{\mathcal {K}}}} \\&= S^{\alpha \gamma }_{\beta \delta }z^*_{\tilde{S},\gamma }(g)z_{\tilde{S}, \delta }(f) \otimes 1_{\tilde{{\mathcal {K}}}} + \delta ^{\alpha }_{\beta } \langle f,g\rangle 1_{\tilde{{\mathcal {H}}}}\otimes 1_{\tilde{{\mathcal {K}}}}\\&= S^{\alpha \gamma }_{\beta \delta }z_{\tilde{S}, \tilde{R}}^*(g_{\gamma }\oplus 0)z_{\tilde{S}, \tilde{R}}(f_{\delta }\oplus 0) + \delta ^{\alpha }_{\beta } \langle f,g\rangle 1_{\tilde{{\mathcal {H}}}}\otimes 1_{\tilde{{\mathcal {K}}}}. \end{aligned} \end{aligned}$$As for (5.7), (5.8), we see that since \(z_{\tilde{S}, \tilde{R}}(f_{\alpha } \oplus 0)\) and \(z_{\tilde{S}, \tilde{R}}(0\oplus g_{\eta })\) operate on different tensor slots they commute. Cyclicity of the vacuum vector is shown in Lemma 5.2, and we note that the annihilation of the normalised vector \(\Omega _{\tilde{S}, \tilde{R}}\) by \(z_{\tilde{S}, \tilde{R}}\) shows that the functional defined by the righthand side of (5.11) satisfies the properties listed in Definition 2.1 and therefore coincides with \(\omega \).

b)
Let \(X\in {\mathcal {Z}}(S\boxplus R, {\mathcal {L}})\). Then
$$\begin{aligned} \begin{aligned} \Vert \pi _{\tilde{S},\tilde{R}}(X)\Omega _{\tilde{S}, \tilde{R}}\Vert ^2&= \langle \pi _{\tilde{S},\tilde{R}}(X)\Omega _{\tilde{S}, \tilde{R}}, \pi _{\tilde{S},\tilde{R}}(X)\Omega _{\tilde{S}, \tilde{R}} \rangle \\&= \langle \Omega _{\tilde{S},\tilde{R}} , \pi _{\tilde{S},\tilde{R}}(X^*X)\Omega _{\tilde{S}, \tilde{R}} \rangle \\&= \omega (X^*X)\\&= \Vert \pi _{\tilde{S}\boxplus \tilde{R}}(X)\Omega _{\tilde{S}\boxplus \tilde{R}} \Vert ^2. \end{aligned} \end{aligned}$$This shows that the map \(V: {\mathcal {P}}_{\tilde{S}\boxplus \tilde{S}}\Omega _{\tilde{S}\boxplus \tilde{R}} \rightarrow {\mathcal {P}}_{\tilde{S}, \tilde{R}} \Omega _{\tilde{S}, \tilde{R}}\), \(V\pi _{\tilde{S}\boxplus \tilde{R}}(X) \Omega _{\tilde{S}\boxplus \tilde{R}} := \pi _{\tilde{S}, \tilde{R}}(X) \Omega _{\tilde{S}, \tilde{R}}\) (\(X\in {\mathcal {Z}}(S\boxplus R, {\mathcal {L}})\) is well defined and isometric. Moreover, for \(X, Y \in {\mathcal {Z}}(S\boxplus R, {\mathcal {L}})\)
$$\begin{aligned} \begin{aligned} V\pi _{\tilde{S}\boxplus \tilde{R}}(X) V^* \pi _{\tilde{S}, \tilde{R}}(Y) \Omega _{\tilde{S}, \tilde{R}}&= V\pi _{\tilde{S}\boxplus \tilde{R}}(X) \pi _{\tilde{S}\boxplus \tilde{R}}(Y) \Omega _{\tilde{S}\boxplus \tilde{R}}\\&= V\pi _{\tilde{S}\boxplus \tilde{R}}(XY) \Omega _{\tilde{S}\boxplus \tilde{R}} \\&= \pi _{\tilde{S}, \tilde{R}}(XY) \Omega _{\tilde{S}, \tilde{R}}\\&= \pi _{\tilde{S}, \tilde{R}}(X) \pi _{\tilde{S}, \tilde{R}}(Y) \Omega _{\tilde{S}, \tilde{R}}. \end{aligned} \end{aligned}$$Since \(\Omega _{\tilde{S}\boxplus \tilde{R}}\) is cyclic for the representation \(\pi _{\tilde{S}\boxplus \tilde{R}}\) and \(\Omega _{\tilde{S}, \tilde{R}}\) is cyclic for \(\pi _{\tilde{S}, \tilde{R}}\), it follows that V extends to a unitary \({\mathcal {F}}_{\tilde{S}\boxplus \tilde{R}}(\tilde{{\mathcal {H}}}\oplus \tilde{{\mathcal {K}}}) \rightarrow {\mathcal {F}}_{\tilde{S}}(\tilde{{\mathcal {H}}}) \otimes {\mathcal {F}}_{\tilde{R}}(\tilde{{\mathcal {K}}})\) satisfying (5.12).
\(\square \)
As a corollary, we note the simple form of Ssymmetrised Fock spaces in the case of S a normal form as previously anticipated.
Corollary 5.4
Let \(S\in R_0({\mathcal {H}})\) be an involutive Rmatrix of normal form (4.4). Then there is a unitary
where \({\mathcal {H}} = \bigoplus _{i=1}^N {\mathcal {H}}_i\).
By the results of [16], we know that any involutive Rmatrix is equivalent to an Rmatrix of normal form. This motivates to ask what we can say about the relation of the Hilbert spaces and the representations of \({\mathcal {Z}}(S, {\mathcal {L}}), {\mathcal {Z}}(R, {\mathcal {L}})\) for two equivalent Rmatrices \(S\sim R\). If they are equivalent, we have unitary intertwiners \(Y_n^{\tilde{S},\tilde{R}}\) (4.3), and their direct sum \(Y^{\tilde{S}, \tilde{R}} = \bigoplus _n Y_n^{\tilde{S}, \tilde{R}}\) defines a unitary \({\mathcal {F}}_{\tilde{S}}(\tilde{{\mathcal {H}}}) \rightarrow {\mathcal {F}}_{\tilde{R}}(\tilde{{\mathcal {K}}})\).
In some cases, this Hilbert space isomorphism also intertwines the actions of the Zamolodchikov operators as we now discuss in two examples.
Example 5.5
Let \(\tilde{S}\in {\mathcal {R}}_0(\tilde{{\mathcal {H}}}), \tilde{R}\in {\mathcal {R}}_0(\tilde{{\mathcal {K}}})\) with \(S\sim R\) (in the type 1 sense) such that we may choose their intertwiner to be of the form
Then
Indeed, we can check by calculation—let \(f \in {\mathcal {L}}\), then by Corollary 4.4 we have the expression \(Y^{\tilde{S}, \tilde{R}} = U^*\left( Y^{S,R} \otimes 1\right) U\) where we note that the intertwiner acts trivially on \({\mathcal {L}}\). This gives
What remains to be shown is to calculate the action of \(Y^{S,R}z_S(e_{\alpha })\left( Y^{S,R}\right) ^*\). Let \(\psi \in {\mathcal {F}}_S({\mathcal {H}})\) then
Thus the adjoint action of \(Y^{\tilde{S}, \tilde{R}}\) results in an isomorphism between elements of the polynomial algebras \({\mathcal {P}}_{\tilde{S}}, {\mathcal {P}}_{\tilde{R}}\).
It must be mentioned, however, that the isomorphism of the Hilbert spaces given by \(Y^{\tilde{S}, \tilde{R}}\) does not always give an isomorphism of Zamolodchikov representations. As a counter example, we restrict to dimension two and consider \(S= F_{{\mathcal {H}}} \sim 1\boxplus 1 = R\). In the Fock representation of \({\mathcal {Z}}(S, {\mathcal {L}})\), we have anticommutation between all annihilation operators, i.e.
for \(\alpha , \beta \in \{1, 2\}\) and all \(f,g \in {\mathcal {L}}\). If an isomorphism between the representations of \({\mathcal {Z}}(S, {\mathcal {L}})\) and \({\mathcal {Z}}(R, {\mathcal {L}})\) existed, this anticommutation would be preserved; however, for some choices of \(\alpha \) and \(\beta \), we actually have commutation in the representation of \({\mathcal {Z}}(R, {\mathcal {L}})\)
for all \(f,g \in {\mathcal {L}}\). A quick calculation shows the product \(z_{\tilde{R}, 1}(f) z_{\tilde{R}, 2}(g)\) is not zero, and thus, the representations \(\pi _{\tilde{S}}, \pi _{\tilde{R}}\) are not isomorphic in this case.
References
Abdalla, E., Abdalla, M., Rothe, K.: Nonperturbative Methods in TwoDimensional Quantum Field Theory. World Scientific, Singapore (2001)
Bostelmann, H., Lechner, G., Morsella, G.: Scaling limits of integrable quantum field theories. Rev. Math. Phys. 23, 1115 (2011). https://doi.org/10.1142/S0129055X11004539
Bratteli, O., Robinson, D.W.: Operator Algebras and Quantum Statistical Mechanics 2. Springer, Berlin (1979)
Baez, J., Segal, I., Zhou, Z.: Introduction to Algebraic and Constructive Quantum Field Theory. Princeton University Press, Princeton (1992)
CastroAlvaredo, O., Fring, A.: From integrability to conductance, impurity systems. Nucl. Phys. B 649, 449–490 (2003). arxiv: hepth/0205076
DuboisViolette, M., Landi, G.: Noncommutative products of Euclidean spaces. Lett. Math. Phys. 108(11), 2491–2513 (2018). https://doi.org/10.1007/s110050181090z. arxiv: 1706.06930
Evans, D., Kawahigashi, Y.: Quantum Symmetries on Operator Algebras. Oxford Science, Oxford (1998)
Faddeev, L.D.: Quantum completely integrable models of field theory. Sov. Sci. Rev. C 1, 107–155 (1980)
Fateev, V.A., Zamolodchikov, A.B.: Conformal field theory and purely elastic S matrices. Int. J. Mod. Phys. A 5, 1025–1048 (1990). https://doi.org/10.1142/S0217751X90000477
Haag, R.: Local Quantum Physics—Fields, Particles, Algebras, 2nd edn. Springer, Berlin (1996)
Jorgensen, P.E.T., Schmitt, L.M., Werner, R.F.: Positive representations of general commutation relations allowing Wick ordering. J. Funct. Anal. 134(1), 33–99 (1995). https://doi.org/10.1006/jfan.1995.1139
Kuzmin, A., Ostrovskyi, V., Proskurin, D., Yakymiv, R.: On \(q\)tensor product of Cuntz algebras. Preprint (2018). arxiv: 1812.08530
Lechner, G.: Polarization free quantum fields and interaction. Lett. Math. Phys. 64, 137–154 (2003). https://doi.org/10.1023/A:1025772304804. arxiv: hepth/0303062
Lechner, G.: Algebraic constructive quantum field theory: Integrable models and deformation techniques. In: Advances in Algebraic Quantum Field Theory, pp. 397–448. Springer (2015). https://doi.org/10.1007/978331921353. arxiv: 1503.03822
Liguori, A., Mintchev, M.: Fock representations of quantum fields with generalized statistics. Commun. Math. Phys. 169, 635–652 (1995). arxiv: hepth/9403039
Lechner, G., Pennig, U., Wood, S.: Yang–Baxter representations of the infinite symmetric group. Adv. Math., p. 106769(2019). https://doi.org/10.1016/j.aim.2019.106769. arxiv: 1707.00196v1
Lechner, G., Schützenhofer, C.: Towards an operatoralgebraic construction of integrable global gauge theories. Ann. Henri Poincaré 15, 645–678 (2014). https://doi.org/10.1007/s000230130260x. arxiv: 1208.2366
Lukyanov, S.: Free field representation for massive integrable models. Commun. Math. Phys. 167(1), 183–226 (1995). https://doi.org/10.1007/BF02099357
Mishchenko, A.V.: On the braided Fock spaces. Ukr. Fiz. Zh. 41, 338–344 (1996). arxiv: hepth/9701192
Murgan, R., Nepomechie, R.: \(q\)deformed \(su(22)\) boundary \(S\)matrices via the ZF algebra. J. High Energy Phys. 6, 2008 (2008). https://doi.org/10.1088/11266708/2008/06/096
Pennig, U.: Exponential functors, Rmatrices and twists. Preprint 4 (2018). arxiv: 1804.05807
Sviratcheva, K., Bahri, C., Georgieva, A., Draayer, J.: Physical significance of \(q\)deformation and manybody interactions in nuclei. Phys. Rev. Lett. 93, 152501 (2004). https://doi.org/10.1103/PHYSREVLETT.93.152501
Scotford, C.: Work in Progress; Ph.D. thesis
Smirnov, F.A.: Form Factors in Completely Integrable Models of Quantum Field Theory. World Scientific, Singapore (1992)
Zamolodchikov, A., Zamolodchikov, A.: Factorized \({S}\)matrices in two dimensions as the exact solutions of certain relativistic quantum field theory models. Ann. Phys. 120, 8 (1979). https://doi.org/10.1016/00034916(79)903919
Author information
Authors and Affiliations
Corresponding author
Additional information
Publisher's Note
Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.
Rights and permissions
Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons licence, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons licence, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons licence and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this licence, visit http://creativecommons.org/licenses/by/4.0/.
About this article
Cite this article
Lechner, G., Scotford, C. Fock representations of ZF algebras and Rmatrices. Lett Math Phys 110, 1623–1643 (2020). https://doi.org/10.1007/s11005020012713
Received:
Revised:
Accepted:
Published:
Issue Date:
DOI: https://doi.org/10.1007/s11005020012713