Quantum spin chains from Onsager algebras and reflection $K$-matrices

We present a representation of the generalized $p$-Onsager algebras $O_p(A^{(1)}_{n-1})$, $O_p(D^{(2)}_{n+1})$, $O_p(B^{(1)}_n)$, $O_p(\tilde{B}^{(1)}_n)$ and $O_p(D^{(1)}_n)$ in which the generators are expressed as local Hamiltonians of XXZ type spin chains with various boundary terms reflecting the Dynkin diagrams. Their symmetry is described by the reflection $K$ matrices which are obtained recently by a $q$-boson matrix product construction related to the 3D integrability and characterized by Onsager coideals of quantum affine algebras. The spectral decomposition of the $K$ matrices with respect to the classical part of the Onsager algebra is described conjecturally. We also include a proof of a certain invariance property of boundary vectors in the $q$-boson Fock space playing a key role in the matrix product construction.


Introduction
The generalized p-Onsager algebra O p (A (1) n−1 ) is generated by b 1 , . . . , b n with the relations where we assume n ≥ 3 and the parameter p is generic. The data (a ij ) i,j∈Zn is the Cartan matrix of the affine Lie algebra A (1) n−1 [14]. The above relation with p = 1 goes back to [28, eqs.(11), (12)]. In what follows, the algebra O p (g) introduced for any affine Lie algebra g [3] will simply be called an Onsager algebra for short. We refer to [27,Rem. 9.1] for the early history of the Onsager algebra starting from [23] and [15,Sec.1(1)] for an account on more recent studies and the references therein.
Let q be a parameter such that q 2 = −p −2 . Then O p (A (1) n−1 ) has a representation b i → b i defined by where z is a spectral parameter and σ ± i = 1 2 (σ x i ± iσ y i ), σ z i are the Pauli matrices acting on the i th component of (C 2 ) ⊗n . Thus the generators of O p (A (1) n−1 ) are expressed as local Hamiltonians of XXZ type spin chain on a length n periodic lattice.
In this paper we explain the origin of the representation (2) and extend it to the Onsager algebra O p (g) associated with the non-exceptional affine Lie algebras 1 g = D (2) n+2 , B (1) n ,B (1) n and D (1) n . It is based on the two recent works; the q-boson matrix product construction 2 of the reflection K matrices connected to the three dimensional (3D) integrability [20] and the characterization of those K matrices by Onsager coideals [19]. The resulting Hamiltonians contain various boundary terms reflecting the shape of the relevant Dynkin diagrams. They yield a systematic realization of the Onsager algebras by spin chain Hamiltonians, providing examples beyond free-fermions which were sought eagerly in the very end of [28].
Let us sketch some more detail of our approach and the results. Our representation of O p (g) is an elementary consequence of the composition 1B (1) n is isomorphic to B n but with a different numeration of the vertices of the Dynkin diagram. See Section 8. It is included for uniformity of the description. 2 The coexistence of p and q related by p = ±iq −1 originates in the q-boson for Up in [20].
where U p (g) denotes the Drinfeld-Jimbo quantum affine algebra [10,13]. The space V is taken as (C 2 ) ⊗n and the latter arrow stands for the fundamental representations for U p (A (1) n−1 ) and the spin representations for U p (g) for the other g mentioned in the above. They carry a spectral parameter z whose dependence is incorporated into b 0 only. (See Remark 3.3 however.) A natural basis of V is parametrized as |α 1 , . . . , α n with α i ∈ {0, 1}, which may be viewed as a state of a spin 1 2 chain with n sites. In this interpretation, the generators e i , f i , k ±1 i of U p (g) are expressed as exchange type interactions among local spins around site i of the lattice. See for instance (51)-(52) for the typical examples in U p (A (1) n−1 ) and also (175), (177) for peculiar ones in U p (D (1) n ) involving "pair creation/annihilation" of two boundary spins. A crux here is to accommodate the length n chain within a single U p (g) module V rather than considering the n-fold tensor product of the spin 1 2 representation of U p ( sl 2 ). Such an approach to size n systems by rank n algebras has also turn out efficient in the mutispecies TASEP [17].
The first arrow in (3) stands for an algebra homomorphism defined by for g = A (1) n−1 . A similar embedding is known for all g [3]. In this context, (1) can be viewed as a modified p-Serre relation. Observe in general that the elements of the form g ′ i = f i + c i k −1 i e i + d i k −1 i ∈ U p (g) with arbitrary coefficients c i , d i behave under the coproduct ∆ (defined in (8)) as It implies that the subalgebra B p ⊂ U p generated by g ′ i 's becomes a left coideal subalgebra ∆B p ⊂ U p ⊗B p . In this vein, the coideal subalgebra of U p (A (1) n−1 ) generated by g i (4) whose coefficients are deliberately chosen to further fit (1) was called an Onsager coideal in [19]. Its natural analogue for g other than A (1) n−1 can also be formulated, albeit that a couple of variants are allowed for the coefficients c i , d i . See (87)-(90) and the remarks following them.
Having the Onsager coideals of U p (g) of a decent origin, it is tempting to seek the associated reflection K matrices governed by them via the boundary intertwining relation [8]. In our setting it is represented as the symmetry of local Hamiltonians where the replacement z → z −1 is relevant only for i = 0. The integer n ′ denotes the rank of g, i.e., n ′ = n − 1 for g = A n−1 and n for the other type under consideration. It was shown in [19] that (5) admits a unique (up to normalization) solution K(z) : V → V satisfying the reflection equation [5,16,25]. Moreover it reproduces the reflection K matrix constructed by the matrix product method connected to the 3D integrability [20]. In other words, these K matrices are characterized by the commutativity with the local Hamiltonians.
Introduce the Hamiltonian H(z) = κ 0 b 0 + κ 1 b 1 + · · · + κ n ′ b n ′ with constant coefficients κ 0 , . . . , κ n ′ . It depends on z via b 0 only. Then (5) implies the quasi-commutativity H(z −1 )K(z) = K(z)H(z) for arbitrary κ 0 , . . . , κ n ′ . In the special case κ 0 = 0, H(z) reduces to a z-independent operator H enjoying the symmetry [K(z), H] = 0. On the other hand, for each g under consideration, we will show that there is one special choice of κ 0 , . . . , κ n ′ (up to overall normalization) such that all of them are non-vanishing and Here K ∨ (z) = σ x K(z) and σ x is the global spin reversal operator (14). In this way, the K matrices in [20] are shown to serve as various versions of symmetry operators of the Hamiltonians consisting of Onsager algebra generators. See also the ending remarks in Section 12.
Our second main result is the spectral decomposition of the K matrices with respect to the classical part O p (g) of the Onsager algebra O p (g) 3 . The former is defined as the subalgebra of the latter by dropping the generator b 0 . The relation (5) tells that K(z) commutes with O p (g) in the representation V under consideration. Therefore it is a scalar on each irreducible O p (g) component within V . We present detailed conjectures on the eigenspectra and the decompositions. A typical formula of such kind is (191). They are boundary analogues of the celebrated spectral decomposition of quantum R matrices with respect to U p (g), and deserve further studies from the viewpoint of representation theory of Onsager algebras.
Our third main result is a proof of Theorem B.1 in Appendix B. It states certain vectors in the qboson Fock space remain invariant under the action of the intertwiner of the quantized coordinate ring A q (Sp 4 ) [18]. The content is apparently independent from the other parts of the paper. However the claim is essential and has been used as a key conjecture in [20] to perform the q-boson matrix product construction of the K matrices for g = D n and D (1) n treated in this paper. So the proof included here really completes the 3D approach by the authors [20] and establishes the reflection equation independently from the representation theoretical method using Onsager coideals [19].
The layout of the paper is as follows. In Section 2, quantum affine algebras U p (g) and the q-boson matrix product construction of the reflection K matrices [20] are recalled. In Section 3, fundamental representations of U p (A (1) n−1 ) are recalled and the Hamiltonian associated with O p (A (1) n−1 ) is given. A simple connection to the Temperley-Lieb algebra [26] is pointed out in Remark 3.1. In Section 4, spectral decomposition of the type A n−1 ) is described. Section 5 is a guide to the subsequent sections devoted to presenting parallel results for O p (g) with g other than A (1) n−1 . It summarizes common and general features in these cases. Concrete formulas for the spin representations of U p (g), Hamiltonians associated with O p (g) and their K matrix symmetry are given in Section 6 for D (2) n+1 , Section 7 for B (1) n , Section 8 forB (1) n and Section 9 for D (1) n . Section 10 and Section 11 describe the spectral decompositions of the K matrices when the classical part of O p (g) is O p (B n ) and O p (D n ), respectively. Section 12 is a summary. Appendix A is a proof of commutativity of the K matrix for type A (1) n−1 . Appendix B contains a proof of the important Theorem B.1. Throughout the paper the parameters q, p are related by (7) and assumed to be generic. We use the notation

General remarks and definitions
In this section we introduce the definitions that will be commonly used in the paper.
n ) (n ≥ 3) be quantum affine algebras without derivation operator [10,13]. The affine Lie algebraB (1) n is just B (1) n but with different enumeration of the nodes as shown in Section 8.1. Note that U p (A (1) 1 ) has been excluded. We assume that p is generic throughout. For convenience set n ′ = n−1 for A (1) n−1 and n ′ = n for the other cases. U p is a Hopf algebra generated by and the Serre relations which will be described later. The Cartan matrix (a ij ) 0≤i,j≤n ′ [14] will also be given later for each case. The constants p i (0 ≤ i ≤ n ′ ) in (6) are p i = p 2 except for p 0 = p n = p for D (2) n+1 , p n = p for B (1) n and p 0 = p forB (1) n . In addition to p, we allow the coexistence of the parameters q, t and the sign factors ǫ, µ related as The second relation is the same with [19, eq.(96)]. The coproduct ∆ is taken as 2.2. U p module V and local spins. We will be concerned with the U p module V with dim V = 2 n presented as Vectors |β with β ∈ {0, 1} n should be understood as 0. The space V will be an irreducible U p module for U p (D n−1 ) and U p (D (1) n ), one needs to introduce the finer subspaces V l and V ± as which leads to the decompositions Let The global spin reversal operator will be denoted by It acts on a base vector as σ x |α = |1 − α where 1 = e 1 + · · · + e n .
2.3. K matrices. Let us recall the matrix product construction of the K matrices related to the 3D integrability [20]. We will not use the reflection equations satisfied by them in this paper. They have been described in detail in [20,19]. Let F q = m≥0 C|m and F * q = m≥0 C m| be the Fock space and its dual equipped with the inner product m|m ′ = (q 2 ; q 2 ) m δ m,m ′ . We define the q-boson operators a + , a − , k on them by They satisfy ( m|X)|m ′ = m|(X|m ′ ) and the relations We also use the number operator h acting as h|m = m|m and m|h = m|m so that k may be identified with q h . Set The K matrix K tr (z) related to U p (A n−1 ) is given by the matrix product formula [20]: The trace here is evaluated by means of (15) and Tr(z h k m ) = 1 1−zq m . All the elements K tr (z) β α is a rational function of z and q. Moreover it is easily seen that K tr (z) β α = 0 unless |α| + |β| = n. Thus (17) is actually refined as K tr (z) = K tr,0 (z) ⊕ · · · ⊕ K tr,n (z), Some examples from n = 3 read which are actually the action of K tr,2 (z). We have slightly changed the gauge in (16) from [20, eq.(6)] and the normalization factor from [20, eq.(77)] to (19) so that is satisfied. Another notable property is the commutativity where [ , ] denotes the commutator defined after (82). A proof of (23) is given in Appendix A.
To present the K matrices K k,k ′ (z) related to U p (D n ), we prepare the boundary vectors Then K k,k ′ (z) are given by the matrix product construction [20]: where the normalization factors are specified as The quantity η k |z h X|η k ′ for any polynomial X in a ± , k can be calculated by using (15) and the explicit formula where θ(true) = 1, θ(false) = 0. Obviously K 2,2 (z) β α = 0 unless |α| + |β| − n ∈ 2Z. Therefore (25) for (k, k ′ ) = (2, 2) is refined as The normalization factors have been chosen so that all the elements of K k,k ′ (z) are rational function of z, q and For instance one has The commutativity (23) does not hold for the K matrices K k,k ′ (z). For later convenience let us introduce two slight variants of the K matrices. The first one is a gauge transformation of K k,k ′ (z) as See (7) for the relation among the parameters q and t. It is symmetric, i.e., In fact, the elementsK k,k ′ (z) β α are obtained from (26) and (27) by replacing the local matrix product operators (16) by a symmetrized one: The second variant of the K matrices is defined by where σ x is the spin reversal operator (14). By the definition their matrix elements are related to the original ones just by As with K tr (z) and K k,k ′ (z), they are linear maps on V . A notable contrast with (20) and (30) is that they now preserve the nontrivial subspaces which exist for U p (A We first present the results for A n−1 case in this section and the next. n−1 ) and fundamental representations. We assume n ≥ 3. The Dynkin diagram and the Cartan matrix are given by The Serre relations have the form and the same ones for f j 's. The fundamental representations are defined on the subspaces V 0 , V 1 , . . . , V n of V in (11) as where z is a spectral parameter. The symbol e j denotes the j th elementary vector This should not be confused with the generator e j of U p .

Onsager algebra
The classical part of A n−1 ) generated by b 1 , . . . , b n−1 is the Onsager algebra for A n−1 . We denote it by O p (A n−1 ). The reason to employ p ±2 here instead of p ±1 is to avoid p ± 1 2 in the forthcoming formulas like (48) and (50)-(52) via q ∓1 by (7).
Remark 3.1. Let T q,n denote the Temperley-Lieb algebra [26] generated by t 1 , . . . , t n−1 obeying the relations Under the relation p 2 = −q −2 according to (7), it is easy to see that yields an algebra homomorphism O p (A n−1 ) → T q,n . The case p 2 = 1 studied in [28] corresponds to the singular situation q + q −1 = 0.
where the latter is the l-th fundamental representation (43) and the former embedding is given by This corresponds to [19, eq.(34)] with p = −iǫq −1 according to (7).
The summands in (50) are expressed by the local spins (13) as follows: The sum of two terms in (51) with i = 0 is also written as where the second summand is a Dzyaloshinskii-Moriya (DM) interaction term. The constant term appearing in (52) will be encountered repeatedly in the sequel. We denote the image of b i by the composition (49) by b i , i.e., b i = π tr l (b i ). Thus it is identified with a local Hamiltonian of XXZ type: The formula (50) corresponds to Its constant shift according to (48), i.e., reproduces the well-known realization of the Temperley-Lieb generators by an n site spin 1 2 chain [24,22,2].
It has been shown [19] that the K matrix K tr (z) (17)-(18) is characterized, up to normalization, by the commutativity with the Onsager algebra: where the replacement z → z −1 matters only for i = 0. Set where the z-dependence comes only from b 0 . We have taken the coefficients of b i 's so that the sum eliminates the σ z i -linear terms in (55), and therefore σ x H tr (z)σ x = H tr (z −1 ) holds with σ x defined by (14). Then (60) and (38) lead to the commutativity To construct higher order commuting Hamiltonians within the Onsager algebra O p (A n−1 ) is an outstanding problem whose solution has been known only at p = 1 [28,4]. See also the ending remarks in Section 12. As far as O p (A (1) n−1 ) is concerned, it may be useful to combine Remark 3.1 and [12]. Let us comment on the hermiticity of the Hamiltonians. The local ones b 0 , . . . , b n−1 (55) are all hermite if and only if |z| = 1 and q ∈ R. When |z| = 1 and q ∈ iR, they are hermite except for the summand 4 The condition a ij = a ji is redundant for A (1) n−1 , but it is included for the later use (91) in non simply-laced algebras.
representing a pure imaginary magnetic field. On the other hand, H tr (z) (61) is hermite if and only if |z| = 1 and either q ∈ R or q ∈ iR. A similar feature holds for g other than A (1) n−1 . Remark 3.3. It is possible to formulate an n-parameter version of the above result. This is due to the algebra automorphism e i → z i e i , f i → z −1 i f i , k i → k i involving the nonzero parameters z i (i ∈ Z n ). Alternatively, one may keep (50) and modify the representation (43) into The choice z i = z for all i ∈ Z n is the model involving uniform DM terms studied in [1]. Introduce K ∨ tr (z 0 , . . . , z n−1 ) = σ x K tr (z 0 , . . . , z n−1 ) similarly to (38), where elements of the latter is defined by generalizing (18) to up to overall normalization. Then the following commutativity is valid: This kind of multi-parameter generalizations are possible also for U p treated in later sections, although they will be omitted for simplicity.

Spectral decomposition of
n−1 ) introduced in Section 3.2 has the representation We denote this restriction also by π tr l . The relation (60) with i = 0 tells the commutativity [K tr (z), π tr l (O p (A n−1 ))] = 0.
The representation π tr l of O p (A n−1 ) on V l is irreducible [19]. On the other hand it is not so with respect to the classical subalgebra O p (A n−1 ). The K matrix K tr (z) should be a scalar on each irreducible component. For instance when (n, l) = (4, 2), it acts on the 4 2 = 6 dimensional space V 2 , and its eigenvalues read The multiplicities 2, 3 and 1 here are equal to the Kostka numbers 4 2 − 4 1 , 4 1 − 4 0 and 4 0 , respectively. Systematizing such investigations leads to the conjecture that there are irreducible O p (A n−1 ) modules W l,j with 0 ≤ l ≤ n 2 or n 2 < l ≤ n having the properties (i), (ii) and (iii) described below: This is consistent with dim V l = n l and satisfies dim W l,j = dim W n−l,n−j . For convenience when n is even, we also define W n 2 ,j with j > n 2 by setting W n 2 ,j = W n 2 ,n−j for all 0 ≤ j ≤ n. (ii) The decomposition K tr (z) ∈ n l=0 Hom(V l , V n−l ) in (20) is refined into K tr (z) ∈ Hom(W l,j , W n−l,n−j ), where each component is an isomorphism of O p (A n−1 ) modules.
(iii) There exists a basis {ξ l,j i | 1 ≤ i ≤ dim W l,j } of W l,j in terms of which the isomorphism in (ii) is explicitly described as the spectral decomposition: We have used infinite products in order to make the formula uniform. However all the eigenvalues of the K matrices appearing here and in what follows are rational functions of z. It is easy to see ρ l,j (z)ρ n−l,n−j (z −1 ) = 1, which is consistent with (22). In view of Remark 3.1, we expect that W l,j (0 ≤ j ≤ l ≤ n 2 ) is the irreducible representation V [n−j,j] of the Temperley-Lieb algebra T q,n labeled with the two row Young diagram [n − j, j] in [11, p126]. The decomposition (70) corresponds to [2, eq.(57)].

5.
Types other than U p (A n−1 ) case in Section 3-4 will be presented individually for the other U p under consideration. They consist of so many cases that one may wonder if it is possible to grasp them in a unified manner. Our aim here is to indicate how to do so at least partially. We note that these variety of cases have originated in the solutions of the reflection equation listed in [20,Sec.6] and the corresponding coideals in [19,App.B].
For convenience we set The superscript r in g r,r ′ indicates that the Dynkin diagram around the 0 th node is an outward double arrow for r = 1 and trivalent for r = 2. The shape around the n th node is specified by r ′ similarly. The quantity p i defined after (6) is written as p 0 = p r , p i = p 2 (0 < i < n) and p n = p r ′ . For each g r,r ′ , we will consider the quantum affine algebra U p (g r,r ′ ) and the Onsager algebra O p (g r,r ′ ) [3]. The Serre relations in U p (g r,r ′ ) read e i e j − e j e i = 0 (a ij = 0), e 2 i e j − (p 2 + p −2 )e i e j e i + e j e 2 i = 0 (a ij = −1), e 3 i e j − (p 2 + 1 + p −2 )e 2 i e j e i + (p 2 + 1 + p −2 )e i e j e 2 i − e j e 3 i = 0 (a ij = −2) (79) and the same ones for f j 's. The other relations have been already given in (6). The Onsager algebra O p (g r,r ′ ) is generated by b 0 , . . . , b n obeying modified p-Serre relations [3]: Except for (79) and (82) which are void for the simply-laced U p (g 2,2 ) and O p (g 2,2 ), these relations are formally the same with those in type A The quartic relation of the form (85) with p 2 = 1 is often referred to as the Dolan-Grady condition [9]. It is typical for the situation a ij = −2, which was indeed utilized to reformulate the original Onsager algebra for A  We will deal with the representations of O p (g r,r ′ ) constructed as π r,r ′ k,k ′ : O p (g r,r ′ ) ֒→ U p (g r,r ′ ) → EndV ((r, k), (r ′ , k ′ ) = (1, 1), (1, 2), (2, 2)) (86) with V = (C 2 ) ⊗n . Thus there are nine cases to consider. We remark that the strange condition r ≤ k, r ′ ≤ k ′ originates in (227) to validate Theorem B.1, which was a key in the 3D approach [20]. The latter arrow in (86) is the spin representations of U p (g r,r ′ ) which will be specified in later sections. They carry a spectral parameter z. The former embedding depends on k, k ′ and is given by See (7) for the relations among the parameters p, q, ǫ etc. Recall also that p 0 , . . . , p n were specified after (6). In general, according to [ provides an embedding O p (g r,r ′ ) ֒→ U p (g r,r ′ ) if and only if the following condition is satisfied: One can check that (87)-(90) fulfills this and the relations (80)-(82) directly. As in U p (A n−1 ), we shall write b i = π r,r ′ k,k ′ (b i ) to mean the representation (86) of b i ∈ O p (g r,r ′ ). Its dependence on (k, k ′ ) should not be forgotten although it is suppressed in the notation for simplicity. Among b 0 , b 1 , . . . , b n , there is a special (affine) one b 0 which includes the spectral parameter z built in the spin representations.
It has been shown [19] that the K matrixK k,k ′ (z) is characterized, up to normalization, by the commutativity with the Onsager algebra: whereK k,k ′ (z) has been defined in (34). It turns out that the analogue of H tr (z) in (61) can be constructed for the representation π r,r ′ k,k ′ if and only if (r, r ′ ) = (k, k ′ ). In fact, for the generators b 0 , . . . , b n in π k,k ′ k,k ′ (O p (g k,k ′ )), it is possible to choose the constant (z-independent) coefficients κ 0 , . . . , κ n so that becomes free from σ z i -linear terms and fulfills σ x H k,k ′ (z)σ x = H k,k ′ (z −1 ). As a result, (92) leads to where K ∨ k,k ′ (z) has been introduced in (38). The concrete forms of H k,k ′ (z) will be presented in (106), (142), (161) and (179).
The local Hamiltonians b 0 , . . . , b n are all hermite if and only if |z| = 1 and t min(k,k ′ ) ∈ R, where t is related to p and q as in (7). When |z| = 1 and t min(k,k ′ ) ∈ iR, some of them acquire a pure imaginary magnetic field term. The Hamiltonian H k,k ′ (z) is hermite if and only if |z| = 1 and either t min(k,k ′ ) ∈ R or t min(k,k ′ ) ∈ iR.
The representations π 1,2 1,2 , π 1,2 2,2 of O p (B (1) n ) on V and π 2,2 2,2 of O p (D (1) n ) on V ± are irreducible [19]. On the other hand they are no longer irreducible with respect to their common classical subalgebra O p (D n ). The K matrices should be a scalar on each irreducible component.
(ii) There exists a basis {ζ ± l,i | 1 ≤ i ≤ dim Z ± l } of Z ± l in terms of which the spectral decomposition of the K matrices is described as where the spaces Y 0 , . . . , Y n are given by C(ζ + n−l,i − ζ − n−l,i ) ( Thus the following relations hold: By the definition the matrix element of K(z)K(w) is expressed as (K(z)K(w)) β1,...,βn α1,...,αn = Tr 12 z h1 w h2 M β1 α1 · · · M βn αn , where the trace extends over the two q-boson Fock spaces 1 and 2. Let r be the exchange operator of the two q-bosons: r 2 = 1, r a ± i = a ± 3−i r, r k i = k 3−i r, rh i = h 3−i r (i = 1, 2).
Appendix B. Proof of the invariance of boundary vectors under 3D K matrix The matrix product construction of the reflection K matrices K k,k ′ (z) in [20] was based on the fact that certain boundary vectors remain invariant under the action of the 3D K matrix K which is the intertwiner of quantized coordinate ring A q (Sp 4 ) [18]. See [20, eq.(78)]. In this appendix we prove this crucial property which had been left as a conjecture in [20], thereby completing the 3D approach there. For simplicity we shall concentrate on the latter relation in [20, eq.(78)] on the ket-vectors. The former relation corresponding to the bra-vector version follows from it by an argument similar to the proof of [18,Prop.2.4]. We leave an detailed description of the 3D K matrix to the original work [18]. A quick exposition is available in [20,Sec.3.2].
Let F q 2 be the Fock space obtained by formally replacing q by q 2 in F q in Section 2.3. The q 2 -boson operators are denoted by A ± , K, i,e,, A − |m = (1 − q 4m )|m − 1 , A + |m = |m + 1 , K|m = q 2m |m .
We introduce the boundary vectors by