Scholarly article on topic 'Conformal higher-spin symmetries in twistor string theory'

Conformal higher-spin symmetries in twistor string theory Academic research paper on "Physical sciences"

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Nuclear Physics B
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Abstract of research paper on Physical sciences, author of scientific article — D.V. Uvarov

Abstract It is shown that similarly to massless superparticle, classical global symmetry of the Berkovits twistor string action is infinite-dimensional. We identify its superalgebra, whose finite-dimensional subalgebra contains psl ( 4 | 4 , R ) superalgebra. In quantum theory this infinite-dimensional symmetry breaks down to SL ( 4 | 4 , R ) one.

Academic research paper on topic "Conformal higher-spin symmetries in twistor string theory"



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Nuclear Physics B 889 (2014) 207-227

Conformal higher-spin symmetries in twistor string


D.V. Uvarov

NSC Kharkov Institute of Physics and Technology, 61108 Kharkov, Ukraine Received 17 June 2014; received in revised form 25 September 2014; accepted 10 October 2014 Available online 16 October 2014 Editor: Herman Verlinde


It is shown that similarly to massless superparticle, classical global symmetry of the Berkovits twistor string action is infinite-dimensional. We identify its superalgebra, whose finite-dimensional subalgebra contains psl(4\4, R) superalgebra. In quantum theory this infinite-dimensional symmetry breaks down to SL(4|4, R) one.

© 2014 The Author. Published by Elsevier B.V. This is an open access article under the CC BY license ( Funded by SCOAP3.

1. Introduction

Twistor string theory [1,2] inspired remarkable progress in understanding spinor and twistor structures underlying scattering amplitudes in gauge theories and gravity. Unlike conventional superstrings the twistor string spectrum presumably includes only a finite number of oscillation modes, in particular those of the open string sector are exhausted by 4-dimensional N = 4 super-Yang-Mills theory and conformal supergravity [3]. Since the latter theory is non-unitary and one is unable beyond the tree level to disentangle its modes from those of super Yang-Mills, there were made over time other propositions of twistor string models [4-6]. However, for tree-level gluon amplitudes there was proved [7] the equivalence of the expressions obtained within the Berkovits model [2] and using the field-theoretic approach. To gain further insights into the properties of twistor strings it is helpful to identify their symmetries both classical and

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0550-3213/© 2014 The Author. Published by Elsevier B.V. This is an open access article under the CC BY license ( Funded by SCOAP3.

quantum. In Refs. [1,8] it was shown that except for an obvious PSL(4\4, R) global symmetry twistor strings are also invariant under its Yangian extension that is closely related to infinite-dimensional symmetry of integrable N = 4 super-Yang-Mills theory [9,10].

In this paper we argue that the world-sheet action of Berkovits twistor string is invariant under infinite-dimensional global symmetry, whose superalgebra contains as a finite-dimensional subalgebra the generators of PSL(4\4, R), 'twisted' GLt(1, R) symmetries and constant shifts of supertwistor components. For the twistor string model with ungauged gl(1, R) current global symmetry algebra is isomorphic to the Dirac brackets (D.B.) algebra of the collection of all monomials constructed from an arbitrary number l > 0 of PSL(4\4, R) supertwistors and the dual supertwistor. We identify this infinite-dimensional superalgebra as a twistor string algebra (TSA). Its finite-dimensional subalgebra is spanned by gl(4\4, R) generators and dual supertwistor corresponding to l = 1 and l = 0 monomials respectively. The relations of the global symmetry algebra of the Berkovits model are obtained from those of TSA by setting to zero gl(1, R) current. In the quantum theory we show that classical inifinite-dimensional symmetry breaks down to SL(4\4, R) one, whose consistency was proved in [8] using the world-sheet CFT techniques.

Infinite-dimensional nature of the symmetries of massless superparticles was revealed already in [11]. So in Section 2 we consider the (higher-spin) symmetries of N = 4 supersymmetric models of massless particles in the supertwistor formulation [12,13]. We included in this section also some of the known material, in particular on the finite-dimensional symmetries and spectrum identification, to make it self-contained and to prepare the ground for subsequent discussion of the twistor string symmetries in Section 3.

2. Higher-spin symmetries of D = 4 N = 4 massless superparticles

Kinetic term of the Shirafuji superparticle model [12] specialized to the case of N = 4 super-symmetry [13] has the form

PSU(2, 2|4) supertwistor ZA has 4 bosonic components Za transforming in the fundamental representation of SU(2, 2) ~ SO(2,4) and 4 fermionic components f' - in the fundamental representation of SU(4) [14]. Components of the dual supertwistor

0 /2x2 2x2 0

transform in the antifundamental representation of SU(2, 2) x SU(4).

In the canonical formulation non-trivial D.B. of the supertwistor components are

{ZA, ZB)d.B. = iSB, {zB, ZA}D.B. = -i(-)asB>

where a is the Grassmann parity equal 0 for the supertwistor bosonic components and 1 for the fermionic components.

2.1. Classical symmetries of D = 4 N = 4 massless superparticle

2.1.1. U(2,2|4) global symmetry

Action (2.1) is manifestly invariant under U(2, 2|4) global symmetry generated by G(1,1) = ZеЛба2 a :

SZA = {ZA, G(i,i) }DB = 1ЛАвZb, 8Za = {Za, G^d.b. = -¡¿вЛБa- (2.4)

Supertwistor ZA and its dual ZA are thus transform linearly under U(2, 2|4). Associated Noether current up to a numerical factor coincides with the generator of U(2, 2|4) transformations and is given by valence (1, 1) composite supertwistor

Tab = ZaZ b (2.5)

that on D.B. satisfies the relations of u(2, 2|4) superalgebra

{Tab, TCD}db = i(SBTad - (-y^sDTcb), sba = (-f+a. (2.6)

Irreducible components of (2.5)

Tab = {T/, Tj; Qaj, Qie; T, U} (2.7)

include the generators of SU(2, 2) x SU(4) transformations, D = 4 N = 4 Poincaré and conformal supersymmetries, U(1) phase rotation and 'twisted' Ut(1) rotation respectively

T/ = ZaZe - 4SP(ZZ), Tj = HiHj - 4sj(HH),

Qaj = ZaHj, Qie = HiZe,

T = Z Z + H H, U = Z Z - H H- (2.8)

Throughout this paper tilde over a tensor indicates that it is traceless under contraction of its upper and lower indices of the same sort. Component form of u(2, 2|4) superalgebra relations (2.6) reads

{T/, Tys}D.B. = i(serTaS - saT/),

{Tj }d.b. = i (KTil - ^),

D.B. M sk Ta ' sa Tk ' 4SiSkT

{Qaj\ QkS }d.b. = i^j TaS + Sa Tkj + 1SlSj T) {Тав, qy1 }d.b. = i(sey Qal - 1 S? Qyiy

{Тав, QkS }DB.. = -i(sl Qkв - \ % Qk*) ,

{Tj qy1 }d.b. = -i(SlQYj - 4Sjqy^ {Tj Qjs }d.b. = Qis - 4sjQj^

{U, Qaj}DB = 2iQaj, {U, Q,e}DB = -2iQie. (2.9)

Few remarks regarding above relations are in order. su(2, 2) © su(4) and supersymmetry generators span psu(2, 2|4) - the minimal superalgebra that includes conformal and ^-symmetries. To obtain in closed form corresponding (anti)commutation relations it is common to set T = 0. The generators of psu(2, 2|4) and T span su(2, 2|4) superalgebra. Unlike the case N = 4 this superalgebra is not simple since T forms an Abelian ideal. Because U does not appear on the r.h.s. of (2.9) u(2, 2|4) superalgebra has the structure of semidirect sum of su(2, 2|4) and ut(1).

Component form of U(2, 2|4) transformations (2.4) is obtained by calculating D.B. of the supertwistor components with the individual generators in (2.8). In such a way we find transformation rules of the supertwistor components under SU(2, 2) x SU(4) rotations

SZa = lAapZp, 8Za = -iZpApa, Aa a = 0;

S? = iAijlj, Sli = -iljAji, Aii = 0, (2.10) supersymmetry transformations

SZa = isail', Sli = -iZaeai;

SZ a = -ilteia, Sli = ie\Za, (ea{ )f = eia, (2.11) as well as, U(1) and Ut(1) rotations

SZa = iaZa, SZa = -iaZa, = ia?, S? = -ia?; (2.12)

SZa = iatZa, SZa = -iatZa, S? = -iat?, S? = iatli. (2.13)

2.1.2. £Sp(8|8) global symmetry

Action (2.1) is also invariant under the symmetries generated by monomials composed of either supertwistors or dual supertwistors only. Linear functions G(i,0) = ZaAa and G(0,i) = AAZA generate constant shifts of supertwistors

SZA = {ZA, G(1,0)}DB. = iAA; SZa = {Za, G(0,1)}d.b. = -iAa. (2.14)

Consider also generating functions defined by valence (2, 0) and (0, 2) supertwistors

G(2,0) = ZA1 Za2 AA2A1 = Za(2)Aa(2) ,

G(0,2) = A A2A1ZA1ZA2 = A A(2)Z a(2), (2.15)

where convenient notation to be widely used below is ZA(l) = ZA1 ■ ■ ■ ZAl (ZA(0) = 1, ZA(1) = ZA) and ZAy) = ZA1 ■ ■ ■ ZAl (ZA(0) = 1, ZZA(1) = ZA)} Associated variations of supertwistors read

SZA = {Za, G(2,0)}db = 2iZBABA;

SZa = {Za, G(0,2)}d.b. = -2iAabZB. (2.16)

Corresponding Noether currents can be identified with valence (2, 0) and (0, 2) supertwistors

Ta(2) = ZA1 Za2 , TA(2) = ZA1ZA2. (2.17)

1 Composite objects like and Za(1) are graded symmetric in their indices. In general it is assumed graded

symmetry in supertwistor indices denoted by the same letters. Similarly one defines the products of supertwistor bosonic and fermionic components as Za(m) = Za1 ■■■Zam, Za(m) = Z a1 ■■■ZZam and !i[n'] = ?i1 •••?in, |]i[n] = ■■■lin (n < N = 4) that are (anti)symmetric. Antisymmetry in a set of n indices is indicated by placing n in square brackets. Both symmetrization and antisymmetrization are performed with unit weight.

Together with u(2, 2|4) currents (2.5) they generate 0Sp(8|8) global symmetry of the Shirafuji model (2.1). (Anti)commutation relations of osp(8|8) superalgebra are given by (2.6) and

{Ta(2), Тв(2) }db = -i ((-r sBjTA1B2 + (-)a2(a1+a2)sB2TA1B1

+ (-)a1(a1+a2)s^Ta B2 + (-y2a2+a1{a1+a2)s^-TA в^

{Ta(2), TbC}d k = -i {(-)a2eCaSC2TA1B + (-)a1^+a2CSCMTA2B), {ta(2), Tbc }db = i(sA2TA1c + (-)a2asA1TA2C ). Decomposition of the generators (2.17)

Tab = {Tap, Tij; Qaj}: Tap = ZaZp, Tij = HiHj,

TAB = {TaP, T!'j ; Qaj } : TaP = Za Ze, Т!;' = H'Hj, allows to find component form of the transformations (2.16) SZa = 2iЛaвZ p ;

SHl = 2iЛaiZa ;

Qaj — ZaHj; Qaj = ZaHj

SZa = -2лшь, SH = -2г'Л%'




8Z a = -2iÀ aPZp ;

SZa = -2iÀ aiSli = -2iÀ aiZa ; 8h = -2iÀ ijlj.

Component form of the relations (2.18) that involve osp(8|8) \ u(2, 2|4) currents reads


{Tap, TyS}db = -iSp TaS + Sp TaY + SY TpS + S*a TpY) - - ^ + S^T + U),

{Tap, QY' }d,b. = -i(SPQal + SlQp1 ),

{Tj, Tkl}d.b. =1 - SjTik - SfT/ + S'j) + 4(S'Sj - SjSj)(Т - U), {Tj, QYl}d.b. = i(SjQiY - SiQ/),

{Qaj, TyS }db = -i (SYQ/ + SSaQ/), {Qaj, Тк%£. = ЩQa' - SjQa"),

{Qaj, QY' }d.B. = i(Sj TaY - SY Т/ + 1 SjSY u)


Accordingly D.B. relations involving both u(2, 2|4) and osp(8l8) \ u(2, 2|4) generators acquire the form

{Tap, V }d,b. = Tap + SaTpy - 1SYTaP^ {Tap, T}d.b. = {Tap, U}d.b. = -2iTap,

{Тaв, QjS}DB = -i{SpQak + SaQpk),

{Tij, Tk' }d.b. = -i(Sj Tik + Si Tkj - 2 Sk "j,

{T;, -T}d.b. = {Tij, U}d.b. = 2iT; {T; Qyl }d.b. = ijn - si Qyj)

{Qy;, V }d.B. = -i ^ Qyj - 4 5Y Q«^' {Qaj, T}D.B. = -2i Qyj, {Qyj, Qyl} d.B. = iSjTay, {Qaj, } D.B. = -iYaT jk,

{Qa;, Tkl }db = -i(&lj Qak - 4 ¿kj (2.23)

{Tyß, fys}DB = i(sßTaS + YyTßs - 4ssY {TУß, T}d.b. = {^ U}d.b. = 2i Tyß,

{Taß, Qy1 }d.b. = i Yy Qal + Y°a Qßl), {T!;, Tkl}d,b. = i(&iT + YkT - 2YkTij

{^ T.d.b. = {T!7, -U.d.b. = {T!j, QkY}d.b. = i (¿IQYl- YkQY;),

lY fD.B.-i\YYQ ~ 4yyq J, lQ , TlD.B

{Qaj, Qrl}d.b. = iYayTjl, {Qaj, QkY}d.b. = iYjTaY,

{Qa;,%Y)d.b. = i(YayQYj - 4yYQy; , {Qa;,TD.B. = 2iQaj,

{Qa;, "Tkl}D.B. = i[YJkQyl - 4 Ylk Qyj ). (2.24)

One observes that the ut(1) generator U appears on the r.h.s. of (2.22) in addition to all the su(2, 2|4) generators. As a digression let us note that OSp(2N|8) d U(2,2\N) symmetry is manifest in the superparticle models [15,16] formulated in generalized superspace with the bosonic coordinates described by symmetric 4 x 4 matrix that in addition to Minkowski 4-coordinates includes 6 coordinates described by the second rank antisymmetric tensor. Lagrangians of these models can be naturally written in terms of orthosymplectic supertwistors transforming linearly under OSp(2N |8).2

2.1.3. Higher-spin symmetries

The complete global symmetry of the model (2.1) is infinite-dimensional. Generic form of the generating function for both finite-dimensional and higher-spin symmetries is

G(t,i) = Zbi ■■■¿BkA*"-Bl M ...a, ZAl • • • ZA, k,l > 0. (2.25)

Parameters AB(k)A(l) (anti)commute with themselves and with the supertwistor components depending on their parities defined by the sum e(A) = Y,k bk + Y,l al of parities bk and al that take

2 String models formulated in terms of OSp(N|8) supertwistors were considered in [17-19]. In Ref. [20] was discussed

their relation to the Berkovits twistor string model [2].

values 0(1) for the indices corresponding to bosonic (fermionic) components of supertwistors. Using associated variation of supertwistors

SZA = {ZA, G(k,i)}DB = ikZs2 • • • ZskABk-B2AC(1)ZC{1),

sZa = {Za, G(k,i)}d.b. = -il^c(k)Ac(k)abl-i-Bi ZBl •• • ZBl-1 (2.26)

one derives the variation of the superparticle's Lagrangian

= (k +1 - 2) — (ZA(k)AA(k)B{i)ZB(l)). (2.27)

From this expression it becomes clear that 0Sp(8|8) symmetry for which (k, l) = (1, 1), (2, 0) or (0, 2) is special since the action is invariant under corresponding variation. For other values of (k, l) the invariance is only up to a total divergence. So the complete infinite-dimensional symmetry of the superparticle model (2.1) is generated by the sum

G = E G(kl) = E ZB(k)AB(k)A(i)ZA(l). (2.28)

k,l>0 k,l>0

Associated Noether currents are given by a collection of all possible monomials of the form

T(kJ)A(k)B(l) = ZA(k)ZB(l), k,l > 0. (2.29)

Such monomials span an infinite-dimensional superalgebra, whose (anti)commutation relations in schematic form read

{T(k,l)B(k)A(l), T{p,q)D(P)C(q)}DB= i(s£ T(k+p-1,l+q-1)B(k)D(P-1)A(l-1)C(q)

- SCT(k+p-1J+q-1)B(k-1)D(p)A(l)C(q-1)). (2.30)

2.2. Quantum symmetries of D = 4 N = 4 massless superparticle

At the quantum level D.B. relations (2.3) are replaced by (anti)commutators3

[ZA, Zb} = SA, [zb, Za} = -(-)asA (2.31)

and components of supertwistors and their duals become Hermitian conjugate operators (Z^ = ZA.4 Thus global symmetry generators are promoted to Hermitian operators. Quantized u(2, 2|4) generators TAB are defined by the graded symmetrized (Weyl ordered) expression

tab = 2 (Za Zb + (-)abZB Z a). (2.32)

As far as component generators (2.7), (2.8) are concerned there are no ambiguities in the definition of su(2, 2) and su(4) generators, because of their tracelessness, and supersymmetry generators, while u(1) and ut(1) generators can be presented in various forms

T = 1 (ZZ + ZZ) +1 (ii - ii) = ZZ + ii = ZZ- ii, (2.33)

U = 2 (Zz + ZZ) - 2 (ii - ii) = zZ- ii+ 4 = ZZ + ii- 4. (2.34)

3 Planck constant is omitted on the r.h.s.

4 Hermitian conjugation is assumed to reverse the order for both bosonic and fermionic operators.

There are no numerical constants in 'asymmetric' representations of T since equal in number bosonic and fermionic components of supertwistor and its dual give contributions that cancel each other. Also no ambiguity arises in the definition of quantized osp(8|8) \ u(2, 2|4) generators (2.17). In general higher-spin generators T(k,l)A(k)B(l) are defined by the sum of all graded permutations of constituent supertwistors

T(kJ)B(k)A(l) = ^ (¿B{k)ZA(l) + ■ ■ ■). (2.35)

They satisfy (anti)commutation relations [21] that in schematic form read

\T(k'l)Bik)A(l), T(p,q)D{p)C(q)}

m<min(l,p) n<min(k,q)

~ XA(m)XC(n)T(k+P-m-n,l+q-m-n) A(l-m)C(q-n) (236)

/ , 0D(m)0B(n) 1 B(k-n)D(p-m) . (2.36)

m,n>0 m+n odd

2.3. Higher-spin symmetries of massless superparticle and higher-spin superalgebras

It is worthwhile to compare considered classical and quantum relations of the higher-spin currents with those of the higher-spin superalgebras based on orthosymplectic symmetries [22]. Generating function (2.28) of the infinite-dimensional global symmetry of the superparticle action (2.1) can be considered as a symbol of the operator G that is defined by the same expression (2.28) in which (Weyl ordered products of) quantized supertwistors (2.31) should be substituted. Associative algebra aq(8|8) (aq = 'associative quantum') of such operators is isomorphic to the *-product algebra of their symbols. The *-product can be brought to the following form in terms of PSU(2, 2|4) supertwistors [21]

A(Z, Z) * B(Z, Z) = Ae B, A = (- dz - - Z, (237)

where A(Z, Z) and B(Z, Z) are symbols of the operators A(Z, Z) and B(Z, Z). Introduction of the Lie superalgebra structure in aq(8|8) requires assignment of parities to the monomials B(k,l)B(k)A(l) (and associated expansion coefficients) in G. The prescription [22] appropriate for the construction of higher-spin gauge theories consists in ascribing parity 1(0) to SU(2, 2) (SU(4)) indices. Such a choice agrees with the spin-statistics relation for the expansion coefficients that are identified with the potentials (field strengths) of higher-spin gauge fields but, for instance, the generators of such a Lie superalgebra defined by the product of an odd number of supertwistor bosonic components should satisfy anticommutation relations, while those equal the product of supertwistor fermionic components - commutation relations. We adhere to alternative prescription motivated by the symmetries of the superparticle action that, however, results in wrong spin-statistics relation for some of the parameters in (2.28). Both prescriptions match for the superalgebras spanned by the generators composed of an even number of supertwistors, in particular for the finite-dimensional symmetries generated by quadratic monomials.

The r.h.s. of (anti)commutators A * B — (-)s(A)s(B)B * A of aq(8|8) elements coincides with that of quantized generators (2.35) so that relations (2.36) can be identified as corresponding to infinite-dimensional Lie superalgebra Lieiaq]^^). Then D.B. relations (2.30) can be identified with the classical limit h ^ 0 of Lie[aq](818) that can be named Lielacl]^^). In general

the classical limit of Lie superalgebras based on *-product associative algebras is obtained by introducing explicit dependence on h

(A * B - (-)e(A)e(B)B * A)(Z, Z) = 1 (AeAB - (-)*(A)*(B)BeA" A),

Ah= h A (2.38)

and taking h ^ 0. h plays the role of the contraction parameter as was explained in [23,22].

2.4. D = 4 N = 4 massless superparticle with gauged U(1) symmetry

Modification of the model (2.1) considered by Shirafuji [12] consists in gauging U(1) symmetry (2.12) by adding T with the Lagrange multiplier to the action

Su(1) = j drXT. (2.39)

Gauging phase symmetry means that superparticle propagates on projective supertwistor space. Global symmetry of the action (2.1), (2.39) is described by a subalgebra of Lie[acl](8\8) spanned by the generators commuting with T. We identify this superalgebra as iuci(2, 2\4). It is the classical limit of iu(2, 2\4) (iu = 'infinite-dimensional unitary') superalgebra introduced in [21]. Both iu(2, 2\4) and iucl(2, 2\4) share the same finite-dimensional subalgebra u(2, 2\4). iucl(2, 2\4) is the centralizer of T in Lie[acl](8\8) analogously to the case of corresponding Lie superalgebras based on associative *-product algebras (see, e.g., relevant discussion in [24]). Generators of iucl(2, 2\4) are the same as those of iu(2, 2\4) and are given by the monomials in (2.29) with equal number of supertwistors and dual supertwistors

T^alb^ - T(LV)B(L) = Za(l)ZB(L), L > 1. (2.40)

Number L we shall call the level of the generator following [25]. D.B. relations of the generators (2.40) can be derived from (2.30)

iT(L1) A(L1) T(L2)T C(L2)\ -¡(XAT(L1+L2-1) A(Ll-l)C(L2)

I1 B(L1) , T D(L2) \D.B. = l\°D1 B(L1)D(L2-1)

_,C T(L1+L2-1) A(L1)C(L2-1))

°B T B(L1-1)D(L2) ).


Going on the constraint shell T « 0 implies setting to zero those generators of iucl(2, 2\4) that are multiples of T. This narrows down higher-spin symmetry to the subalgebra of iucl(2, 2\4). For N = 4 such a symmetry is generated by the classical limit of isl(2,2\N) superalgebra [21]. The construction of this superalgebra is based on the direct sum representation of u(2, 2\N) as su(2, 2\N) © TN5 and its higher-spin generalization. The N = 4 case requires special treatment since su(2, 2\4) = psu(2, 2\4) © T4.

2.5. Spectrum identification

Important realization [26,12] of quantized (super)twistors related to the definition of twistor wave functions is to treat components of ZA as classical quantities, while components of the dual supertwistor ZA are considered as differential operators

5 In this and some of the subsequent formulas to avoid confusion T is endowed with the subscript explicitly indicating the number of odd components of associated supertwistors.

" dZa ' d§

acting in the space of (homogeneous) functions of (Z, §). Alternatively, components of Za may be treated as c-numbers, while components of Za are replaced by differential operators.

Quantum generator (2.33) of ^(1) phase symmetry in the realization (2.42) can be brought to the form

T = 2s + 2 - § — , (2.43)

where s = -1 - 1 Zd is the helicity operator [27]. Any homogeneous function on the su-pertwistor space is its eigenfunction including the wave function F(Z, §) of the superparticle propagating on the projective supertwistor space that satisfies

s+ 1 - 2§d)F(Z,§) = 0■ (2.44)

The solution to this equation is

F(Z, §) = f(Z) + %\Pi(Z) + i§i[2]fi[2](Z)

+ 3 §'[3]pm(Z) + 4y §ll4]ft[4](Z). (2.45)

Even components in the expansion f, f [2] and f [4] upon the twistor transform [27] describe bosonic particles of helicities -1, 0 and +1 on (complexified conformally-compactified) Minkowski space-time, whereas odd components Pi and pi[3] - fermions of helicities -1/2 and + 1/2, altogether forming D = 4 N = 4 super-Yang-Mills multiplet that is CPT self-conjugate, i.e. includes particles of opposite helicities.

The spectrum of the superparticle model (2.1) is described by an infinite series of even F2k(Z, §) and odd @2k+i(Z, §) (k e Z) eigenfunctions of the operator (2.43)

1 d a \

s+ 1 - ^ ^ + -2) Fa(Z,§) = 0:

f(s+ 1 - 1 + k)F2k = 0, a = 2k,

\ - 1 a 1 (2.46)

|(s+ 1 - 2+ k + 2)02k+1 = 0, a = 2k + 1, y J

where the subscript indicates homogeneity degree. Pairs of functions Fa and F-a (a > 0) describe (upon the twistor transform) CPT conjugate doubleton supermultiplets [28,29] with helicities ranging from -a/2 - 1 to a/2 + 1 that are even6 for even values of a and odd for odd values of a. This explains the notation introduced in Eq. (2.46). The low-spin supermultiplets in this series are with particles of helicities 0, ±1/2, ±1, ±3/2 and F±2 describing D = 4 N = 4 Einstein supergravity. The only exception is F0 = F twistor function corresponding to the self-conjugate super-Yang-Mills multiplet considered in the previous paragraph.

Another way to derive the spectrum [13] of the superparticle model (2.1) is to transform [30,31] supertwistor components into two pairs of bosonic and two pairs of fermionic SU(2) oscillators realizing [SU(2)]4 - the maximal compact subgroup of SU(2, 2|4). They provide

6 The supermultiplet is even/odd if the particle with the highest value of the modulus of helicity is boson/fermion.

minimal (single generation) oscillator realization of the su(2, 2\4) superalgebra and are used to construct doubleton supermultiplets [32,28,29]. All these supermultiplets assemble into two singleton supermultiplets of osp(8\8) that arise upon quantization of the massless superparticle on superspace with bosonic 4 x 4 matrix coordinates [16].

3. Higher-spin supersymmetries in twistor string models

For Lorentzian signature world sheet the simplest twistor string action can be presented as S = j dxdo(LL + Lr):

Ll = -2(Yad-Za + md-Hl) + LL-mat, Lr = -2(Yad+Za + nid+li) + LR-mat,

where d± = 2 d ± da), a± = t ±a, Y+a = Ya, Y-a = Ya, n+i = ni, n-i = ni and LL(R)-matare Lagrangians for left- and right-moving non-twistor matter variables, whose contribution to the world-sheet conformal anomaly equals c = c = 26 to cancel that of (b, c)-ghosts. Such variables may contain a current algebra for some Lie group (see, e.g., [3]). In Berkovits twistor-string model [2] global scale symmetry for both left- and right-movers

SZa = AZa, &Ya = -AYa, 8? = A?, 8m = -Am;

8Za = AZa, 8Ya = -AYa, 8li = Ali, 8m = -Am (3.2)

is gauged by adding to the action (3.1) appropriate constraints T = YaZa + ni^ 0 and T = YaZa + ni^ 0 with the Lagrange multipliers

sgl(1,W) = j dTda (XT + IT). (3.3)

This necessitates add two units to the central charges of the matter variables to compensate that of (b, c)-ghosts and ghosts for the gauged GL(1, R) symmetry.

Definition of the open string sector, that to date is the only one well-understood, is based on the conditions ZA = ZA, YB = YB imposed on the world-sheet boundary on the supertwistors ZA = (Za, ZA = (Za, li) and their duals Yb = (Yp, nj), Yb = (Yp, nj). So taking into account reality condition of the Lagrangian one is led to consider left(right)-moving supertwistors ZA (ZA) and dual supertwistors YB (YB ) as independent variables with real components. Such supertwistors are adapted for the description of fields on D = 4 N = 4 superspace for the spacetime of signature (+ +---).7 Conformal group of Minkowski space-time of such a signature is

SO(3, 3) ~ SL(4, R) and its minimal N = 4 supersymmetric extension is PSL(4\4, R) with the bosonic subgroup SL(4, R) x SL(4, R) implying that bosonic and odd components of ZA belong to the fundamental representation of SL(4, R)L x SL(4, R)L, whereas bosonic and odd components of YA belong to the antifundamental representation. Correspondingly components of ZA and YA transform according to the (anti)fundamental representation of SL(4, R)r x SL(4, R)r .8

7 Detailed discussion of the reality conditions of the twistor string Lagrangian for both Lorentzian and Euclidean world sheets, and different real structures in the complex supertwistor space associated with D = 4 space-times of various signatures can be found, e.g., in [4].

8 In this section the same letters are utilized to label supertwistors, their components and indices as in the previous one, although here they are strictly speaking different mathematical objects related to another real structure in the complex

Focusing on the sector of left-movers of the model (3.1) and applying the Dirac approach yields equal-time D.B. relations

{Za(a),Yp (a >)}Db = 8p(a - a'), {?(a), (a '))ов = 8)8 (a - a') (3.4)

that in terms of the PSL(4\4, R) supertwistors can be written as

{ZA(a), Ув(а')}DK = 8AB8(a - a'),

[Ув(а), ZA(a')}DB} = -(-)a8B8(a - a'). (3.5) Similar relations hold for the right-movers.

3.1. Classical symmetries of twistor strings

Global symmetry of the left-moving part of the action (3.1) is generated on D.B. by the function

G = f daJ2GL)(a), G(L)(a) = Ув^)Лв al...Ai ZAl (a)■ ■ ■ ZBL(a). (3.6)

For arbitrary value of the order L transformation rules for the supertwistors read

8Z A(a) = ЛА b(l)Z B(L)(a),

8YB(a) = -LYc(a )ЛС abl-lB ZBl (a)... Z Bl-1 (a). (3.7)

Associated Noether current densities up to irrelevant numerical factor are given by the monomials

T(L)BA(L)(a) = УвZA(L), L > 0 (3.8)

that enter generating functions G(L). On D.B. they generate the TSA9

{T(L)BML)(a), T(M)DC(M){a')}DB = (8AT(L+M-1)BA(L-1)C(M)

- 8cT(l+m-1)DA(L)C(M-1))(a)8(a - a

The finite-dimensional subalgebra of TSA is spanned, apart from the order 0 generator yA(a) that is responsible for constant shift of the supertwistor components, by quadratic monomial in supertwistors

TAB(a) = УaZ B, (3.10)

generating gl(4\4, R) superalgebra

supertwistor space. For the dual supertwistor and its components we use independent notation since quantities with bars are reserved to label variables of the right-moving sector of the twistor string. We hope this will not cause a confusion since in each section only one kind of supertwistors is considered.

9 To be more precise one has to introduce TSA as an infinite-dimensional Lie superalgebra and then consider its loop version pertinent to twistor-string global symmetry. Let us also note that the subscript L in the notation of symmetry groups and algebras will be omitted as the discussion is concentrated on the sector of left-movers only. On the boundary left- and right-moving variables are identified and thus also no subscripts are needed.

— I8B T. D — ( — \°b°d '

cb — (_\a+b

{TaB (a), TcD(a')} DB. = (8bTaD - (-)*& 8DATcB)(a)8(a - a'),

B°a = (-)"+b- (3.11)

Irreducible components of gl(4\4, R) current densities (3.10) are TAB(a) = {Tap, Tij; Qaj, Qip; T, U}:

Tap = YaZp - 18pp(YZ), Tij = - 18j(n%);

Qaj = YaHj, Qip = niZp; T = YaZa + , U = YaZa - . (3.12)

The densities of sl(4, R) x sl(4, R) currents Tap(a), Tij (a) and those of the supersymmetry currents Qaj(a), Qip(a) span psl(4\4, R) superalgebra, while these generators and T(a) span sl(4\4, R). On D.B. they generate infinitesimal SL(4, R) x SL(4, R) rotations of the supertwistor components

8Za(a) = Aa pZp (a), 8Ya(a) = -Yp(a)Apa, Aaa = 0; 8? (a) = Aij^j(a), 8m(a) = -nj(a)Aji, Aii = 0 (3.13)

and supersymmetry transformations

8Za(a) = eai?(a), 8m(a) = -Ya(a)eai;

8Ya(a) = -m(aWa, 8? (a) = jaZa(a), (3.14)

where eai and e'a are independent odd parameters with 16 real components each. T(a) generates GL(1, R) transformations (3.2) and U(a) - 'twisted' GLt(1, R) transformations

8Za(a) = AtZa(a), 8Ya(a) = -AtYa(a),

8? (a) = -At?(a), 8m(a) = Atm(a). (3.15)

gl(4\4, R) relations (3.11) are spelt out in terms of irreducible components (3.12) as

{Tap(a), TyS(a')}db = - 8SaTyp)(a)8(a - a'),

{Tij(a), Tk\a') }DB = (8jfil - 8\Tkj)(a)8(a - a'),

{Qaj(a), Qk8 (a ')}d,b. = j8 + 8%j + 18j^(a)8(a - a'),

{Tap(a), Qyl (a ')}db, = (8pqJ - 18pQyl^(a)8(a - a'),

{Tap(a), Qk8(a')}D^ = -(8lQkp - 48pQk^(a)8(a - a'),

{Tij(a), Qyl (a ')}E)^ = ^8ltQYj - 4 8j QYl^j(a)8(a - a'),

{Tij(a), Qk8 (a ')}d,b. = (&1 Qi8 - 4 8jQk^(a)8(a - a'), {U(a), Qaj (a ')}DB = 2Qaj (a )8(a - a'),

{U(a), Qip (a ')}DB} = -2Qip(a)8(a - a'). (3.16)

T (a) commutes on D.B. with all other gl(4l4, R) current densities thus forming an Abelian ideal. The density U(a) of 'twisted' glt(1, R) current does not appear on the r.h.s. of (3.16) that allows to consider gl(4l4, R) as the semidirect sum of sl(4l4, R) and glt(1, R).

3.2. Quantum symmetries of twistor strings

It was shown in [8] that SL(4l4, R) symmetry is preserved at the quantum level, whereas the generator U of 'twisted' GLt(1, R) symmetry has anomalous OPE with the world-sheet stress-energy tensor implying that corresponding symmetry is broken in twistor string theory. Thus possible type of infinite-dimensional symmetry that could survive in the quantum theory is restricted to that based on sl(4l4, R) as finite-dimensional subalgebra. Since gl(4l4, R) superalgebra belongs to the family of gl(MlM, R) superalgebras, whose properties differ from those of gl(MlN, R) superalgebras with M = N, one is forced to take components of supertwistors as building blocks of the generators for sl-type superalgebras.

3.2.1. Superalgebraic perspective on quantum higher-spin symmetries

In the bosonic limit TSA reduces to TSAb - an infinite-dimensional Lie algebra, whose generators are obtained from (3.8) by setting to zero fermionic components of the supertwistors. Order 0 and 1 generators are given by the dual bosonic twistor Ya and gl(4, R) generators YaZ$. The latter divide into sl(4,R) T/ and gl(1,R) T0 = YaZa ones. Higher-order generators YaZ^(L) divide into

Proceeding to TSA superalgebra, from (3.9) one infers that the D.B. relations of order L and M generators close on order L + M - 1 generators. So that order 1 generators, i.e. gl(4l4, R) ones (3.12), play a special role: D.B. relations of the generators of an arbitrary order L with those of order 1 yield again order L generators. This feature can be used to characterize irreducible higher-order generators.

Thus the form of irreducible order 2 generators can be found by D.B.-commuting corresponding bosonic generator (3.17) with order 1 supersymmetry generators and Qaj, dividing generators that appear on the r.h.s. into irreducible SL(4, R) x SL(4, R) tensors, then D.B.-commuting them with Q^ and Qaj and so on. In such a way we obtain

T/(L) = YaZ?(L) --L-(Y Z)S^(1) Zp(L-l)


and T0Z@(L . Expression (3.17) is an obvious generalization of T/ from (3.12) to the case L > 1.

{Qi^(a), TyS(2)(a ')}db, = (s^S(2) - 5 Sp Q^2 ^^(a)S(a - a %


QtS(2) = niZS(2)


D.B.-commutes with . Analogously calculation of D.B. relations of TY&(T> and Qaj yields

{■QaJ(a), TyS(2){a')}DBi =-(sSS T/2)J - 1S^1 QaS2)jya)8{a - a'), (3.20)

where another order 2 supersymmetry generator

QySl = TYS*i


D.B.-commutes with Qaj. Applying Qaj to QkS(2) gives {QaJ(a),QkS(2)(a')}DB = SJkTaS(2\a)S(a - a')

+ S(S1 (TkS2)j + S]k(40T - ^^ZS2^(a)S(a - a')


and similarly

{Q.^(a), QySl (a ')}DB = (sPfS - 1 SsYfiP^(a)S(a - a ')

fvPS + ( — T - — U Y + 1 40 40

S?ZS - i sz

(a)S(a - a'), (3.23)

Ti0j = TijZ0. (3.24)

Continuing further one recovers the set of irreducible order 2 generators

T 0(2) T aj T j[2] - Y [2]-

Ta i Ti , Ta — 1 as ;

Qia(2), Qa0j, T1l2] = mS112] - 1 (nS)sj1 (3.25)

TZa, UZa, T§i, U§i. (3.26)

The operators associated with the generators (3.26), as will be shown below, are not the primary fields in the world-sheet CFT and hence corresponding symmetries are broken at the quantum level. Since these generators appear on the r.h.s. of (3.22), (3.23) this implies breaking of the order 2 supersymmetries Qia(2), Qa0j and, in view of (3.18), (3.20) breaking of the bosonic symmetry generated by TYS(2). So that classical order 2 symmetries break in the quantum theory.

For order L > 2 calculation of D.B. relations of the corresponding bosonic generator (3.17) and order 1 supersymmetry generators gives

0(a) T «»(a = fa™ - -L ^ y

{Qi^(a), TyS(L)(a')}DM = (&PQiS(L) - ^Ssy(1)QiS(L-1)^(a)S{a - a'), (3.27)

{Qaj(a), fYS(L)(a >)}d.k = - Ssa(1)fyS(L-1)j - ^ Ssy(1) faS(L-1)^(a)S(a - a %


where order L supersymmetry generators are defined by the expressions

QiS(L) = mZS(L), fyS(L-1)j = fyS(L-1)*j. (3.29)

Their D.B. relations with order 1 supersymmetry generators read

{QaJ(a), Qk8(L)(a')}D,B, — 8jfa8(L)(a)8{a - a') + 8s™

kl 8(L + 3)' 8(L + 3)



(a)8(a - a ')


{Q,p(a), QyS(L-1) (a ')}dbB, = ^ Tl8(L-1)l - L±2 ^ Tlp8(L-2)l^(a)8(a - a ')

TvmL-i) ± ( _±±1_t -^Z-Lu

8(L ± 3)

x (8pZ8(L-1) -—88v(1)ZpZ8(L-2) Y L ± 2 Y

8(L ± 3) (a)

x 8 (a - a '),

8(L-1)j = TklZ8(L-1)



Continuing further calculation of D.B. relations of gl(4\4, R) supersymmetry generators and order L generators allows to find complete set of irreducible order L bosonic

T P(p)j[q]- T v(p)pj[q]

Ta — Ta S ,

fP(p)j[q] = Tj [q] zp(P), and fermionic generators

TaP(p)j[q] = TJ,{p)s,j [q],

Q.P(p)j[q] = Q.j [q ]ZP(p)^

f — 0, 2, 4, p ± q — L; — 1, 3, p ± q — L

q — 1, 3, p ± q — L; q — 0, 2, 4, p ± q — L.



Relevant (traceless) products of bosonic components of supertwistors are defined in (3.17) and the definition of (traceless) products of fermionic components is given in (3.12), (3.25) and by the expressions

t [3]=L3j -- (nmj1 j t 2i

Qi = m, Qij [4] = mtj [4]. There are also generators of the form

TZa(p)ti[q], UZa(p)ti[q], p > 0, 0 < q < 4. (3.36)

It is these generators that correspond to non-tensor operators in the world-sheet CFT. They are present on the r.h.s. of (3.30) and (3.31) implying breaking of order L symmetries in analogy with those of order 2.

In Berkovits twistor string theory GL(1, R) symmetry is gauged so that generators carrying the factor of T are set to zero. However, GLt(1, R) symmetry, being anomalous, cannot be gauged thus the generators carrying the factor of U cannot be put to zero. So we conclude that for any order L it is not possible to find a set of generators with closed D.B. relations that would correspond to the primary fields. As a result the quantum symmetry of the twistor string reduces to SL(4\4, R) x SL(4\4, R) for the sector of closed strings and its diagonal subgroup for the sector of open strings.

[j1 tj2 tj3]


3.2.2. Higher-spin symmetries from the world-sheet CFTperspective

This subsection we devote to consideration of the twistor part of the left-moving world-sheet CFT justifying the arguments above discussion relied on. To apply the 2d CFT technique to the model (3.1) it is helpful to carry out Wick rotation to Euclidean signature world-sheet

t ^ ia2, a ^ a1 ^ a +^ z = a1 + ia2, a~^-z = -{a1 - ia2).


The following changes of the world-sheet derivatives

d+^ dz = 2(d1 - id2) = d, d-^-di = --d + id) = -d, (3.38)

2d volume element

dTda ^ ida 1da2 = -d2z, (3.39)

and supertwistor components

Ya ^ Ya(z) , Ya ^ - Ya(z) , (3.40)

result in the Euclidean action

v2„(^ . 5 crA , ,

Jd 2z(YAd Z A + YAd Z A). (3.41)

Non-trivial OPE's for the supertwistor components of the left-moving sector, on which we focus,

Za (z)Yp(w)--Si(z)nj(w)--J— (3.42)

z - w z - w

in terms of the supertwistors can be written as


Za(z)Yb(w)--Yb(z)Za(w) --L-L-B. (3.43)

z-w z-w

By definition primary fields are characterized by the following general form of the OPE with the world-sheet stress-energy tensor

L(z)O(w)--^rO(w) + dO(w), (3.44)

(z - w)2 z - w

where h is conformal weight of the primary field.10 The supertwistor part of the left-moving stress-energy tensor for the twistor string model (3.1) equals

Ltw(z) = -YAd ZA (3.45)

so that YB and ZA are primary fields of conformal weight 1 and 0 respectively.

From the world-sheet CFT perspective the necessary condition for the considered global symmetries to survive in the quantum theory is that their generators become primary fields, i.e. their OPE's with the stress-energy tensor are anomaly free, in other words, on the r.h.s. of (3.44) there

10 It is assumed that composite operators depending on a single argument are normal-ordered but normal ordering signs : : will be omitted.

should not appear terms with poles of order higher than two. As we find the generators containing the factor of T or U fail to comply with this requirement. Using the relations

Yy dZY (z)Yp Za (w) - P - ---YpZa(w) - ---d{YpZa)(w) (3.46)

(z - w)3 (z - w)2 (z - w)

nkdf(z)n^(w) - - Sj - 1 m?(w) - —d {ng)(w), (3.47)

(z - w)3 (z - w)2 z - w w '

it follows that sl(4\4, R) generators TaP, Tij, Qa j, QiP and T are primary fields of unit weight, while U is not [8]

-8 1 1

Ltw(z)U(w) - --- + ---U(w) +-dU(w). (3.48)

(z - w)3 (z - w)2 z - w

Higher-order generators (3.33), (3.34) also become primary fields of unit weight. While OPE's of the generators (3.36) with the stress-energy tensor are anomalous

Ltw(z)TZa(p)^i[q](w) - - P + q3 Za(p)^i[q](w) + O{(z - w)-2)

(z - w)3

Ltw(z)UZa(p)%i[q\w) - -8 + P -Za(p>^i[q](w) + O{(z - w)-2). (3.49)

(z - w)3

In the case p = q = 0 one recovers discussed above OPE's of gl(1, R) and glt(1, R) generators with the stress-energy tensor. For p = 0, q = 0 anomalous terms do not vanish so that associated symmetries are broken. Since generators (3.33), (3.34) are linked with other order L generators by order 1 supersymmetries (cf. Eqs. (3.27)-(3.31)) it appears that higher-spin symmetry is broken for arbitrary value of L except for L = 1, for which quantum-mechanically consistent global symmetry is isomorphic to SL(4\4, R).

4. Conclusion and discussion

In this paper we performed the analysis of higher-spin global symmetries of D = 4 N = 4 massless superparticle models in supertwistor formulation extending the consideration of Ref. [11]. Discussed infinite-dimensional conformal superalgebras stemming from the ag(8\8) algebra require further study as they could underly N = 4 supersymmetric extension of interacting higher-spin theories on AdS5 [33,34] and conformal higher-spin theories on D = 4 Minkowski space-time [35]. We have also revealed inifinite-dimensional classical symmetries in the Berkovits twistor string model and its extension with ungauged GL(1, R) symmetry. Noether current densities associated with these symmetries have been constructed in terms of PSL(4\4, R) supertwistors. In the generalized twistor string model the D.B. relations of the Noether current densities have been shown to form the TSA inifinite-dimensional Lie superalgebra, whose finite-dimensional subalgebra is spanned by gl(4\4, R) generators and the generator of constant shifts of the supertwistor components. The full classical symmetry of the twistor string action is generated by the direct sum of two copies of TSA superalgebra for the left- and right-movers that for the open string sector are identified on the boundary. Classical symmetry of the Berkovits model is described by the subalgebra of TSA obtained by going on the constraint shell YaZa + ni^ 0.

Its finite-dimensional subalgebra is spanned by psl(4l4, R), 'twisted' glt(1, R) generators and that of shifts of the supertwistor components.

The fact that the symmetry of twistor string action is infinite-dimensional is anticipated due to the symmetry enhancement in N = 4 super-Yang-Mills theory at zero coupling [36,37]. One could similarly anticipate infinite-dimensional symmetry of free N = 4 conformal supergravity [38] that is present in the spectrum of Berkovits twistor string on equal footing with N = 4 super-Yang-Mills theory. Observed infinite-dimensional symmetry breaking down to SL(4l4, R) at the quantum level also agrees with the higher-spin symmetry breaking in N = 4 super-Yang-Mills once the interactions are switched on [37]. Looking at the symmetry enhancement on the stringy side [36,39] in the weak coupling regime of gauge/gravity duality our results seem to support the evidence [20] for the tensionless nature of twistor strings or rather certain equivalence of the limits of zero and infinite tension [40]. Interesting question is whether other twistor string models [4-6] are invariant under higher-spin symmetries.

To conclude let us make a few comments on the twistor string spectrum. There are three kinds of states in the open string sector of the Berkovits model [3]. Twistor counterpart of N = 4 super-Yang-Mills multiplet is described by the vertex operator

Vym(Z) = Jr(Z)Fr(Z (Z)), (4.1)

where jR (R = 1,..., dimG) represent currents of unit conformal weight from the current algebra G that enters the Lagrangian LL(R)-mat in (3.1) and FR(Z) is a scalar function on the supertwistor space of homogeneity degree zero. Other options to construct vertices of overall conformal weight one and homogeneity degree zero are

Vf(z) = yA(z)fA(Z (z)), Vg(z) = ea(Z (z))d ZA (4.2)

with the supertwistor functions fA(Z) and gA(Z) having homogeneity degrees (GL(1, R) charges) +1 and -1. They satisfy the constraints dAfA = ZAgA = 0 and are defined modulo the gauge invariances SfA = ZAf, SgA = dAg to match upon the twistor transform the states of N = 4 conformal supergravity [3]. As far as the open string sector of the model (3.1) is concerned the vertex operators are formally remain the same as above but the condition of zero homogeneity degree in supertwistor components is relaxed so that FR(Z) describes not only N = 4 super-Yang-Mills states but also all the doubleton supermultiplets via the pairs of functions F±a(Z) having opposite homogeneity degrees +a and -a. In particular, functions F±2(Z) describe N = 4 Einstein supergravity multiplet. It is then natural to take jR corresponding to some Abelian algebra. The states of N = 4 Einstein supergravity also reside in conformal supergravity vertices (4.2) with the supertwistor functions constrained by the ansatz fA(Z) = IABdBF+ 2(Z) and gA(Z) = F-2(Z)IabZb, where IAB, Iab are infinity supertwistors [41]. Supertwistor functions fA(Z) and gA(Z) with other values of GL(1, R) charges correspond to higher-spin counterparts of N = 4 conformal supergravity multiplet and deserve further study. In the Berkovits twistor string model important role is played by the gauged GL(1, R) symmetry that allows to shift conformal weights of the supertwistor fields and reproduce scattering amplitudes for various helicity configurations of external particles. In the ungauged case to be able to study scattering amplitudes of particles from, for instance, doubleton supermultiplets some additional variables should be introduced. This could impose further restrictions or lead to the determination of the structure of yet undetermined matter Lagrangians in (3.1).


The author is grateful to A.A. Zheltukhin for stimulating discussions.


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