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Nuclear Physics B 886 (2014) 712-732

www. elsevier. com/locate/nuclphysb

Massive spin-2 in the Fradkin-Vasiliev formalism. I. Partially massless case

Yu.M. Zinoviev

Institute for High Energy Physics, Protvino, Moscow Region, 142280, Russia Received 30 May 2014; accepted 13 July 2014 Available online 16 July 2014 Editor: Stephan Stieberger

Abstract

We apply Fradkin-Vasiliev formalism to construction of non-trivial cubic interaction vertices for massive spin-2 particles. In this first paper as a relatively simple but instructive example we consider self-interaction and gravitational interaction of partially massless spin-2.

© 2014 The Author. Published by Elsevier B.V. This is an open access article under the CC BY license (http://creativecommons.org/licenses/by/3.0/). Funded by SCOAP3.

1. Introduction

Last years there were a lot of activities in the investigation of consistent cubic interaction vertices for higher spin fields. Such investigations are very important steps in the search for consistent higher spin theories and, in particular, provide information on the possible gauge symmetry algebras behind such models. Till now most of the results were devoted to cubic vertices for massless higher spin fields and now we have rather good understanding of their properties. Moreover, the results obtained by different groups and different methods are perfectly consistent, see e.g. [1-10].

At the same time investigations of cubic vertices containing massive higher spin fields are not so numerous, the most important one being classification of cubic vertices in flat Minkowski space by Metsaev [11-13], while there also exist a number of concrete examples e.g. [14-24].

E-mail address: Yurii.Zinoviev@ihep.ru. http://dx.doi.org/10.1016/j.nuclphysb.2014.07.013

0550-3213/© 2014 The Author. Published by Elsevier B.V. This is an open access article under the CC BY license (http://creativecommons.org/licenses/by/3.0/). Funded by SCOAP3.

One of the approaches that turned out to be very effective for investigation of massless higher spin fields interactions is the Fradkin-Vasiliev formalism [25,26] (see also [27-30]). Let us briefly remind how this formalism works. The basis for the whole construction is the framelike formalism [31-33], where massless higher spin particle is described by a set of (physical, auxiliary and extra) one forms that we will collectively denote as $ here. As far as the free theory is concerned, three most important facts are:

• Each field has its own gauge transformation

S$ - Df © ef

where D is (A)dS covariant derivative, while e is background (A)dS frame;

• Gauge invariant two-form (curvature) can be constructed for each field

R — D A $ © e A $

• Free Lagrangian can be rewritten in an explicitly gauge invariant form

L0 - ^ R a R

Using these ingredients cubic interaction vertices can be constructed by the following straightforward steps.

• Take the most general quadratic deformation for curvatures

R = R © $ A $

as a result, these new deformed curvatures ceased to be invariant:

SR- $ A Df © e A $f

• Introduce corrections to gauge transformations

S$ - $f in such a way that

SR- D A $f © e A $f

• Adjust coefficients so that deformed curvatures transform covariantly

SR- Rf

• At last, consider the Lagrangian in the form

where the first part is just the sum of free Lagrangians with initial curvatures replaced by the deformed ones, while the second part contains all possible abelian vertices. By construction and due to Bianchi identities, all variations for such Lagrangian take the form

SL - R A Rf

reducing the problem to the set of algebraic equations. Moreover, Vasiliev has shown [34] that for the three massless fields with arbitrary spins s1, s2 and s3, all non-trivial cubic vertices having up to s1 + s2 + s3 - 2 derivatives can be constructed in this way.

As we have seen two main ingredients of this approach are frame-like formalism and gauge invariance. But frame-like gauge invariant description exists for massive higher spin fields as well [35-39]. Thus it seems natural to extend Fradkin-Vasiliev formalism to the cases where both massive and (partially) massless fields are present. Such approach has already been successfully applied to the investigation of gravitational and electromagnetic interactions for simplest massive mixed symmetry field [40,41]. Now we are going to apply this approach to the construction of cubic vertices for massive spin-2 particles.1 In this first paper we restrict ourselves with relatively simple but instructive case of partially massless spin-2 field [42-45] leaving general massive case for the second part.

The paper is organized as follows. In Section 1 we illustrate general approach on the simplest but physically important example of massless spin-2 field in (A)dS space. Namely, we consider both self-interaction as well as gravitational interaction vertices for such field. The main Section 2 is devoted to the partially massless spin-2 case. First of all in Subsection 2.1 we provide all necessary kinematic formulas. Then in Subsections 2.2 and 2.3 we consider self-interaction and gravitational interaction correspondingly. Due to the presence of zero forms as well as a number of identities making different terms equivalent on-shell, an analysis turns out to be more complicated than in the purely massless case. Thus as an independent check for the number of non-equivalent cubic vertices (as well as very instructive comparison) in Appendix A we reconsider the same vertices in a straightforward constructive approach.

1.1. Notations and conventions

We work in (A)dS space with dimension d > 4 with (non-dynamical) background frame and (A)dS covariant derivative DM normalized so that

[Dß,Dv]$a = -K(eßa$v _ eva$ß), k —-

(d - l)(d - 2)

Here Greek letters are used for the world indices, while Latin letters denote local ones. As it common for the frame-like formalism, all terms in the Lagrangians will be completely antisymmetric on world indices and we will heavily use notations like

— e ae b e be a

2. Massless case

2.1. Kinematics

In the frame-like formalism free Lagrangian for massless spin 2 field in (A)dS background has the form:

M ^X^acbc M »val , abn u c (d _ 2)k i »v K b 2 abr» œv _ 2 abc\°^ ^--— ab

This Lagrangian is invariant under the following gauge transformations:

1 Let us stress that we consider massive spin-2 as a simple representative of massive higher spin fields, and not as massive graviton.

8oo^ab = D^fjab + Ke^afb],

'->! — Din ~rKeiA, f , Soh^a = D^fa +ijiia It is easy to construct two gauge invariant objects (linearized curvature and torsion):

RiVab = D[iOv]ab + Ke[i^ahv]b] Tiva = D[ihv]a - 0[i,v]a

Differential identities for them look like:

0n ab _ _Ke [aT b] D T a _ _n a

[lRva] — Ke[i Tva] , D[iTva] — R[iv,a]

Note that on mass shell for auxiliary field oiab we have

Tiva & 0 ^ R[iv,a]a & 0, D[iRva]ab & 0 The free Lagrangian can be rewritten in the explicitly gauge invariant form:

I !vaP\ R abR cd a 1

L0 = a0j abcd\Riv , a0 = — 32(d - 3)k

2.2. Self-interaction

The most general quadratic deformations for curvatures have the form:

AR^vab = b00[icaOv]bc + bih[iahv]b AT^va = b20[iabhv]b If we require that deformed curvatures transform covariantly we have to put:

bi = Kb0, b2 = b0

In this case corrections to the initial gauge transformations look like

Soab = b0[oic[af]c + Kh^afb]]

4~abi b i abtbl

-n hi + oi f \ while deformed curvatures transform as follows:

ab tb]

SRivab = b0Rivc[anb]c + Kb0Tiv lafb]

STiva = -b0nabTivb + b0Rivabf Let us consider the following Lagrangian

L = «{

abn cd i \lvaPY\n ab n cd, e Rat +c0) abode] Riv Rat hY

where the first term is just the free Lagrangian where initial curvature is replaced by the deformed one, while the second term is an abelian vertex. Using identities given above it is easy to check that both terms are gauge invariant on-shell. This Lagrangian gives the following cubic vertex (here and in what follows the second index denotes the number of derivatives in the vertex2):

2 Calculating the number of derivatives we take into account that auxiliary field Oiab is equivalent to the first derivative of physical field.

Li = Li4 + Li2 + L

Li4 = -8aobo\y ^ } D^avabaaceapde + 4co j ^bcdl] D^ab Daa>pcdhYe L12 = 8k(aobo + 2co(d - 4) J DaOvabha^ d

- 16aobo(d - 3)k | 'tla [ h^aavbdaacd

j j I DUav ha

Lio = 16(d - 3)k2(aobo + co(d - 4)) ^ h/hvbhac

Thus we have two independent vertices with terms up to four derivatives.3 But on-shell we have

f /¿VaPy\ abn^ cd, e ^ } Iivap\ ab ce„ de

4CM dbcde I D^^v Damp hy « 12c^ ^^ [ D^ m>a mp

- 8c0(d - 4)k { Ha} [2miadmvbdhac + miabmvcdhad ]

Thus if we put

all four derivative terms cancel on-shell leaving us with the vertex containing no more than two derivatives:

Li = bo 1 2

i^Val ad bdu c 1 \ „ abh ch d

| abc J a ^ av ha - 2 j abcd\D'a h* hP

(2d - 5)k f jxva

huahvbh c

3 j abc fhI hv ha

2.3. Gravitational interaction

For the second spin-2 we will use notations (^Iab, f^a), (nab, Ha) and (Fivab, Tiva) for fields, gauge parameters and gauge invariant curvatures correspondingly.

Let us consider gravitational interactions for this second spin-2. Similarly to the previous case for the deformations of gravitational curvatures we obtain

AR^vab = bo[ n^nvb + ffv]b]

AT„va = bo^[^abfv]b (11)

while deformed curvatures will transform as follows:

8R„vab = boF^vc[aVb]c + KboT^v laSb]

8T»va = -bonabTv + boF,vabe (12)

3 We are working in the linear approximation so for any two solutions their arbitrary linear combination is also a solution. Thus the number of independent solutions is just the number of free parameters.

As for the deformations for the second spin-2 curvatures they correspond to standard minimal substitution rules for gravitational interactions:

AF^ab - bil^a^ + fH v]b] while transformation rules for them look like

AT,^ = bi [^abhv]b + a^fv]b] (13)

sF^vab - bi[-i,claF,J]c + kT^vlaib] - nclaR,J]c + KT„v[aHb]\

8%va = bi l-W + F^vabkb - na%vb + R^vabHb] (14)

Note that at this stage two parameters b0 and bi are independent and it may seem that it contradicts with the universality of gravitational interactions. The reason is that covariance of deformed curvatures guarantees that equation of motion for the theory we are trying to construct will be gauge invariant but it does not guarantee that these equations will be Lagrangean. Thus if we put these deformed curvatures into the Lagrangian and require that this Lagrangian be invariant we have to expect that parameters b0 and bi will be related. As we will see right now it turns out to be the case.

Let us consider the following Lagrangian:

„ I I i-^. ab -£ cd I n ab n cd] , „ I HvaPY I t- ab t- cd i e no

L = a°\ abcd J ^ Fap + R^v Rap \ + ci( abcde j Fap hY (i5)

where the first two terms are just the sum of free Lagrangians with initial curvatures replaced by the deformed ones, while the last term is an abelian vertex. Note that there is one more abelian vertex

\r r- \ ^vapY\ -r ab n cd f e AL = c2( abcde J Rap fY

but (as we have explicitly checked) this vertex completely equivalent on-shell to the one with coefficient ci so we will not introduce it here. Let us take transformations of curvatures that do not vanish on-shell:

SF^vab - -bilncla F^vb]c + nclaRv]c ]

SR^vab - -boncla F^vb]c (i6)

Variations under the nab transformations trivially vanish on-shell, so let us consider the ones for the nab transformations:

IAV(Xp \ ^ tt ab d _ce^de , u TT ae d .bc^de~\

-4ao ^ [bi^vabRapcende + boF^vaeRapbcnde]

But on-shell we have two identities

\^vapY\ aR bcde_ 2\ V-vaP\T ael R be ncd Rabcnde]

0 abode] F»v>a Rap n - 2\ abcd] L-Rap n - Rap n J

0 & J lxvaPY \ -T ab-n cnde _ 2 I ^vaP I It- aen bencd -p abn cende]

0 abcde] -ap,Y n - 2( abcd] n - n J

and their combination gives us

{ IZd] [FivabRapce + FivaeRapbc ]nde « 0 (17)

Thus we have to put (as expected)

bx = b0 (18)

So, as in the previous case, we have two independent vertices with free parameters b0 and c1 and terms containing up to four derivatives. Let us extract all the terms for the cubic vertex:

A = L14 + £12 + L10

£14 = -8a0b0 { IbaP} [2Di^vabnacempde + D^mvab Vace ttpde] + M Ibfdy}D^vabDa^cdhye

£12 = -8a0b0K(d - 3) j Iba} №i/dttvbd + 2^iadMvbd fac]

+ 8k { Ibad] [(2a0b0 + 2(d - 4)c1)Di^vabfachdd + ^^D^fa" fpd ]

£10 = 16k2(d - 3)(3a0b0 + (d - 4)d) | ^ 11 fvb-hac

But on the auxiliary fields mIab and fiiJ,ab mass shell we have

4^ Tcdye}D^vabDaVdcdhye

« 4c1 { Ibbad] [2Di^vab^acempde + Dimvabnacettdde]

- 4K(d - 4)^ Ibad} [2D^vabfachdd - Dimvabfacfdd ]

thus for c1 = 2a0b0 all four derivative terms vanish leaving us with the vertex containing no more than two derivatives:

£1 = T { 7ba} №iad^vbd + 2^iadmvbdfac ]

ab c d ab c d

b0 i iivap

4 ( Zcd\ [2DlAabfachpd + Dimvabfacfdd]

(2d - 5)Kb0 ' iva 1 f,afvbhac (19)

3. Partially massless case

3.1. Kinematics

In the frame-like formalism gauge invariant description for the partially massless spin-2 particle [35,39] requires two pairs of (auxiliary and physical) fields: (^iab, f^a) and (Bab, Bi). Free Lagrangian for such particle has the form:

2 I Z - 2 Г Vf + 2 Bb — ^ -ab.

Z\<bBv + eßaBabfßb

where m2 = (d - 2)к. This Lagrangian is invariant under the following gauge transformations:

Soß/b = Dßnab, Sofßa = + nßa +

(a — 2)

S0Bab = -mnab, SoBц = Drf + 2it (21)

Correspondingly, we have four gauge invariant objects (curvatures):

F,vab = D^]ab _ (j—)e^aBv]b]

T^va = D[^fv]a _ + _ 2) e[^aBv]

= D,Bab + mn^ab

Btv = D[tBv] _ Btv _ — f[t,v] (22)

They satisfy the following differential identities:

D т ,ab -_m_er [aR b

D[tFva] = j _ 2)e[^ Bv,a]

D[tTva] = _F[tv,a] _ j _ 2) e[t Bva]

D[^Bv]ab = mFUvab

D[^Bva] = _B[t,va] _ 2T[tv,a] (23)

Note that on mass shell for auxiliary fields Htab and Bab we have

Ttva & o, Btv & o ^ F[tv,a]a & o, B[t,va]^ 0

Using these curvatures the free Lagrangian can be rewritten in an explicitly gauge invariant form

£0 = °l{ taZd] FtvabFaeCd + Я2 { tl] B,/CBvbC + a3 j ^ } B„abTvaC (24)

16(d _ 3) 1 1

———ai _ a2 = т—j, a3 = _-7— (d _ 2) 2m2 4m

The ambiguity with coefficients is related with the identity

J tvae\ г abK cd 1 J flvaP[ |- ab n K cd , n -r abK cd

0 = ) abcd\DtiFva B \ = j abcd ( DaBP + DtFva BP J

mi iivafi] ab cd 8m(d _ 3) f

\ n acn bc

= abcd] Ftv Fae + (d _ 2) \ab\ Bt Bv

In what follows we will use the convenient choice

ai = —;

(d — 2)

32 (d — 3)m2' 3.2. Self-interaction

a.2 = —■

a3 = —

Following general procedure we begin with the most general quadratic deformations for all four curvatures:

Milvah = dinl^clanv]b]c + d2B^aBv]b] + d3BabB„v + d4efaBb]cBv]c + d5ei^aev]bBcdBcd + d6^abBv] + d1B[l^fv]b] + dgBabfi^,v] + d9e^aBb]cfvf + dfafv]b]

AT^a = dii^abBv]b + di2 Bab^v]b + di3e[^a^v]DcB

a r? bc z>bc

+ di4tt[^abfv]b + di5B[^a Bv] + di6f[^aBv] ab

AB,ab = di7tt,c[aBb]c + dnBabB

ABMv = di9B[^a fv]a

Usual requirement that deformed curvatures transform covariantly gives solution with five arbitrary parameters. However, due to the presence of zero form Bab there are four possible field redefinitions (their explicit action can be seen in Appendix A):

ttuab ^ Q,r + KiBabB^, Ua ^ f/ + K2BabfMb + K3BabB^b + K4e^aBbcBb

* f T ~ Cf + IK. Uf, J f — J f

Using this freedom we can bring the deformations into the form

a bc bc

AF,vab = di

tt[Mc[attv]b]c +

(d — 2)

(B[MiaBv]b] — e[M[aBb]cBv]c)

O ab n Rabn dab f

Bv]--B bmv — B J[M,v]

ATtlva = 2ditt[Mab fv]b

I ¡¡v

ABMab = ditt[Mc[aBb]c — d6BabBi

M B — d6B BM

Mv = —diB[x

ABxv = —diB[Mafv]a

d6 = —

(d — 2)

This corresponds to the following gauge transformations for the deformed curvatures:

&Pxvab = 2diFxvc[anb]c + | B[xab^v] + d6Fxvabï 8%va = —2dmabTxvb + 2diFxvabf 8Bxab = —dinc[a Bxb]c + d6BxabÇ

&BMv = —diB[M,v]"^a

Now let us consider the following Lagrangian:

г л [ ßvaß\ f. abf- cd \ acn bc , „ \ ßVa\ £ ab-f- c

L = ai) abcd] ^V FFaß + a2\ab\B* Bv + abc j B* Tva

+ «{ Zf/e] ^abF«ßcdf/ + «{ Z) B*ad Bvbdfac

+ Tcß} F*vabBacdBß (28)

Here the first line is just the free Lagrangian where initial curvatures are replaced by the deformed ones, while the second line contains possible abelian vertices.4

Let us require that this Lagrangian be gauge invariant. All nab variations vanish on-shell. For the * variations we obtain

2(d—4^04 ma6\ i*vaß\ abT cdb 2d6a1 + (d — 2) +—)\abcd] Fß *

+ (2d6a2 + 2mas + ^^^ { ^ } B^B^ = 0

(d — 2) J [ab Thus we have to put

2(d — 4)ma4 mae

2d6ai + —-)-4 +-6 = 0 (29)

(d — 2) 2

8(d — 3)ma6

2dea2 + 2ma5 +--———— = 0 (30)

(d — 2)

For the transformations we get

I т- ad ю bcs-d

(4d6ai + mae + 2d№) j VB* ?

+ (— mb)|T ) VB,bd4c

and using on-shell identity

o ^ aZd] Bpbc^d={ aia}j,ivad \--2B«bd^c+Bbcïd \ (31)

we obtain

16(d — 4)ma4

8d6ai + 2ma6 + 4da +---mas = 0 (32)

(d — 2)

Thus we obtain three equations which uniquely determines all free coefficients a4,5,6 so we have one cubic vertex with terms up to four derivatives. Note that the case d = 4 is special because the term with coefficient a4 is absent. Happily the solution still exists, namely

as =--2 ' a6 = ^ T—2

m2 2m2

Moreover, as we have explicitly checked, all cubic terms with four and three derivatives vanish on-shell and we reproduce rather well known two derivative vertex [14,46,47]. Note also that the

4 Note that in the partially massless case (and in the massive case too) due to peculiarities of gauge transformations the

terms in the second line are not gauge invariant separately.

same general results (one four derivative vertex in d > 4 and one two derivative vertex in d = 4) was obtained also in [22].

3.3. Gravitational interaction

We begin with the most general quadratic deformations for gravitational curvatures:

ARfvab = b!^ifcla^v]b]c + b2Bi![aBv]b] + b3BfvBab + b4efaBb]cBvf + b5eifaev]bBcdBcd

\fabBv] + b7Bifa fv]b + b&B"1 Jif,v] if

+ b6QifabBv] + b7Bi![afv]b] + b&BabfifM + b9en^aBb]cfv]c + bwfi![afv]b]

ATfva = bn^i!abfv]b + bi2fi!aBv] (33)

The solution has the form (again using all possible field redefinitions):

b6 b6 2b i b2 =--, b3 =--, b4 =--, b5 = 0

4m m (d - 2)

2mbi b6 b6 2mbi

b7 = ———— — —, b8 = ^ —, b9 = --

(d - 2) 2' 2' (d - 2)

m2bi mb6 4mbi

bio =----, bii = 2bi, bi2 =--+ b6

10 (d - 2) 4 ' 11 1 12 (d - 2) 6

Gauge transformations for the deformed curvatures look like:

8Rfvab = 2b1Ffvcianb]c - b6Bfvnab + b7B[fJae] - hB^^] - b9efa Bv]b]cSc + 2b1oTfv ia^b] + b6Ffvab^

'fv S + b6F fv

sfv = -2b1nabTfvb + 2b1FfvabSb - b12BfvSa + buTfvaS (34)

As for the partially massless curvatures deformations they again correspond to the minimal substitution rules:

AFfvab = -boM[!cia^v]b]c + [B[flaK]b] - en[aBb]chv]c]

ATfva = -bo^nabfv]b - bo^nabhv]b - -2mb0rhi!aBv]

(d - 2)'

- (d - 2)

ABfab = -bo^!cvaBbc

ABfv = boBi!ahv]a + m-° fi!ahv]a (35)

while their transformations have the form:

SFF!vab = -boF!vcianb]c - boR!vcianb]c + 7-^ b] + ei!laBv]b]cSc]

(d - 2)

8%va = bonabT!vb - boF!vabSb + T2^B!vSa

(d - 2)

+ bona%vb - boR!vabSb - -dm\T!vaS

(d - 2)

sBtab = _bo Btc[anb]c

ЯК h К ata I mbo TT aZa mb° ^ ata

Stt^v = boB[t,v] S +--— F^v S--— Tfv S

Now let us consider the following Lagrangian:

I tvafi I -г abr cd . „ I fv I n ac n bc

L = abcd] Ftv Fae + a2[ ab] Bt Bv

ab^- c . „ ) tvafi\ n abn cd T va + ao i , , f Rfv R-aB

Тс \ Bta"Tvac + a°\ abcd \ K»v'" Rae

f tlviceY\ -г abT cd, e , „ \ fva 1 „ ad K bd, c

+ °4 1 abcde I ^f Fee hY + j abc | Bf Bv ha

{¡лусв 1 abcd J

ab cd Rfv Ba Be

Here the first line is the sum of the free Lagrangian for partially massless and massless spin-2 where initial curvatures are replaced by the deformed ones, while the second line contains possible abelian vertices. Note that one more possible term

f tvaeY \ -r ab„ cd f e [abcde] Ftv Rae fY

is on shell equivalent to some combination of others so we will not introduce it here.

Now let us require that this Lagrangian be gauge invariant. All nab variations vanish on-shell so we begin with \a transformations. We have to take into account the part of variations that do not vanish on-shell, namely

SF,vab = B[tMlaSb], S%va = _boFtvabSb

(d _ 2)

This produces:

16m[(d _ 4)a4 _ aibo] (d _ 2)

Using on-shell identity i jxvap 1

five abc

ad bd c

tv BabaSc _ a3bo\ fbC] FivaaBabcS

ad bc d с

Ffvad[ _2BabdSc + BabcSd]

0 abcd] ^^ Bpbc^d - 1 abc \">"v

we obtain first equation:

i6l(d - 4)a4 - aib0] , b0

--as +--r- — 0

(d - 2) 2m2

For the nab transformations we have to take into account only

SRfvab = 2b1Ffvcvanbic, This gives us

ab ce de

c[a nb]c

SFivab = _boR,

c[a^b]c

{fivap 1

using once again on-shell identity (17) we obtain

4°1bo\ ZCd] FtvabRaecende _ 8aob1 J ^ J Fivae nbe RaPcd

a1bo + 2aob1 = o (39)

Non-vanishing on-shell part of the Sa transformations has the form

8R!vab = b7B!v][aSb] - b&B[!abSv]' 8%va = -boR!vabSb and we get

-(a3bo + 8aobs - ma6) \ R!vadBabcSd - 16^7 ^ 1 R^BabdSc

Using on-shell identity (31) (where F!vab is replaced by R!vab) we obtain

a3bo + Saobs - ma,6 + 8aob7 = o (4o)

At last let us consider variations under S transformations:

8R!vab = b6^!vabS This produces

2aob6 + 2

f !vafi\ ab„ cdt [abcd] F!v RaP S

and we obtain the last equation

4aob6 + ma.6 = o (41)

These equations have the following solution

bo 16(d - 4)a4

b1 = ^ —' b6 = 2mbo, a5 = ————--16aobo' «6 = -8aobo (42)

2 (d - 2)

Thus in general d > 4 case we have two independent vertices with parameters bo and a4.5 In d = 4 the parameter a4 is absent leaving with one vertex only. Moreover, we have explicitly checked that in this case all four derivative terms vanish on-shell. Note that, contrary to the self-interaction case, here our results do not agree with the one obtained in [22]. Table "2-2-2 couplings" in Appendix B of [22] gives four non-trivial vertices: two four derivatives ones and two vertices having no more than two derivatives. Moreover, these results do not depend on space-time dimension. Due to very different approach used by authors of [22] it is not an easy task to see where and why such difference arises.

4. Conclusion

As we have seen application of Fradkin-Vasiliev formalism to the partially massless (and even more so in the massive) case appears to be more complicated and less elegant. The reason is that due to the large number of fields (main and Stueckelberg) and due to the presence of zero forms one faces a lot of ambiguities related with non-trivial on-shell identities and field redefinitions. Nevertheless, the formalism does work and allows one to obtain reasonable results.

5 As it will be shown in Appendix A in d = 3 case there exists one more cubic vertex with no more than two derivatives, but Fradkin-Vasiliev formalism we use here works in d > 4 dimensions only so we did not obtain such vertex here. Note also that in a frame-like gauge invariant formalism this vertex has been constructed in [2o].

Acknowledgements

Author is grateful to R.R. Metsaev and E.D. Skvortsov for useful discussions. The work was supported in part by RFBR grant No. 14-o2-o1172.

Appendix A. Partially massless spin-2 in a constructive approach

In this appendix as an independent check for the results obtained in the main part we reconsider the same problems in the straightforward constructive approach.

A.1. Modified 1 and | order formalism

In the constructive approach one usually assumes that the action can be considered as a row in the number of fields:

S = So + S1 + S2 + ...

where So is free (quadratic) action, S1 contains cubic terms, S2 - quartic ones and so on. Similarly for the gauge transformations one assumes:

S$ = So$ + S1$ + S2$ + ...

where So is non-homogeneous part, S1 is linear in fields and so on. Then variations of the action under any gauge transformations can also be represented as a row:

SSo /5S1 SSo \

SS = isSo$ + SSo$ + SS1&) + ... S0 \S0 S0 J

First term simply implies that the free action So must be gauge invariant under the initial gauge transformations 8o@. Thus the first non-trivial level (that we will call linear approximation) looks as:

5Si SSo

—18o$ + -S ¿1$ = o

Working with the frame-like formalism it is convenient to separate physical $ and auxiliary Q fields. Than in the honest first order formalism one has to achieve:

5Si 5Si SSo SSo

—So$ + — SoQ + —oS1$ ^ —°S1Q = o S $ o S Q o S $ 1 S Q 1

It means that one has to consider the most general ansatz both the cubic vertex as well for the corrections to gauge transformations for the fields $ and Q. Taking into account that equations for auxiliary fields are algebraic and on their mass shell these fields are equivalent to the derivatives of physical ones, in supergravities there appeared a so-called 1 and 2 order formalism. Schematically it looks like:

TSrSo$ + TsrS1$ $ $

S (So+Sj)_ o S Q =o

So one needs the most general ansatz for cubic vertex and physical fields gauge transformations only, but all calculations have to be done up to the terms proportional to the auxiliary fields equations, i.e. on their mass shell. Such approach turned out to be very effective, but it requires

explicit solution of non-linear equations for auxiliary fields that can be rather complicated task. If we restrict ourselves with the linear approximation than there exists one more possibility that we will call modified 1 and 2 order formalism. It looks like:

8Si 8S0

—180$ + —1+ —0 81$ 80 8Ü 8$

The main achievements here are twofold. At first, we have not consider the most general ansatz for cubic vertex but terms that are non-equivalent on auxiliary fields mass shell only. At second, we need explicit solution for the free auxiliary fields equations only. In what follows we will use such modified formalism.

A.2. Self-interaction

Our aim here is to determine the number of independent vertices so to simplify calculations in this and subsequent subsections we will heavily use all possible field redefinitions and all existing on-shell identities. We will work in an up-down approach i.e. we begin with four derivative terms, then we consider terms with three derivatives and so on.

Vertex 2-2-2 with four derivatives

The only (on-shell non-trivial) possibility here is:

L14a = ao j abcd

Vertex 2-1-1 with four derivatives The most general6 ansatz looks like:

„b J [aitt„abDvBcdBcd + a2V„acDvBbdBcd + a3V„ac DvBcd Bbd

+ aAV„cdDvBabBcd + asQ„cdDvBacBbd + a6,Q„cd DvBcd Bab ] But we have three possible field redefinitions:

f„a ^ f„a + KlBabB„a + K2e„aB2 B„ ^ B„ + K3V„abBab and two on-shell identities (up to lower derivative terms):

^ J D^Üv/BabBcd = J ^ J Dlxnvcd [BabBcd - 2BacBbd] ^ J Ü^cd[DvBabBcd - 4DlBacBbd + DvBcdBab] 0 ^ { Ted] ^!abDvBapBcd = 2J ^J [^iabBcd - 4^iacBbd + i2icdBab]DvBcd

Thus we have one independent vertex only in agreement with fact that there exists only one cubic 2-1-1 vertex with three derivatives for the massless fields. In what follows we will use

6 Up to the terms that are equivalent on-shell.

Li4b = ai\ IXaVb\D^vcdBacBbd

Vertex 2-2-1 with three derivatives

Here the most general ansatz has the form:

Li3 = ( ^ 1 [biDittvabBcdfad + b2DittvadBbdfac + b3Di^vadBbcfad]

+ { ab } [b4^Iab^VcdBcd + b5^acVvcdBbd]

First of all note that in this case we have one possible field redefinition

fia ^ fia + K4Babfib and one on-shell identity (again up to the lower derivative terms)

0 ^ !bafd] D^v,aaBbcfpd = j la) D^vad [Bbcfad — 2Bbdfac ]

Moreover, it is easy to check that invariance under the Ça transformations requires b2 = —2b3, so the terms with the coefficients b2,3 vanish on-shell, while the one with coefficient b1 can be removed by field redefinition.

Collecting all things together let us consider the following cubic Lagrangian:

Li = ao j Ibfd\ Di^vabnacenpde + ai J ^ D^ BacBbd

+ J Ob] [b4 ttiabttvcdBcd + b5^iac^vcdBbd ] (A.i)

nab transformations produce the following variations for this Lagrangian:

SoLi = 2m(d— 24})a0{ ab" 1 [Di^vabBcdncd — 4D^vacBcdnbd]

2m(d — 4)a0 Bcd^ab — 2maiBac^bd (d — 2) 1 i n

+ { av\ [b4DiBcd {ttvabncd — Vvcdnab) + b5 DiBac(ttvbdncd — ttvcdnbd )] — m\ j [b4^oab^vcdncd + b5 ^iac^vcdnbd ]

The terms in the first line can be compensated by the following corrections to gauge transformations:

S1f!a = a1Babmb + a2 nabB!b + «3«/ (Bn) while for the second line we use on-shell identity

o « D!Qv adBadnbc = { ^ J D!Qvcd [Bcdnab - 2Bacnbd] and obtain

2(d - 4)a0

1 (d - 2)

The remaining terms cannot be compensated by any corrections to gauge transformations so we have to put

b4 = b5 = 0

Thus we get rather simple vertex with four derivatives. But such vertex exists in d > 4 dimensions only, while it is well known that in d = 4 there exists cubic vertex having no more that two derivatives. So we proceed and consider the following ansatz:

r I nva\ ad n bd f c , „ J ''vaP[ n n ab f c f d

Ll = ci( abcj^ fa + C2( abcd\D'^v faf

+ cse^aB2f^a + C4 {'va abc} UaBbcDvBa

+ di j IXaVbac\ n,/bBvfac + d^ ^ UaBbcfvc (A.2)

ia transformations produce the following variations:

{ 'aba] [—(2ci + 4c2)D^vadVabdic - 2c2D^vabnacdid ]

(+"OlT j

+ e'a[-(2c3 + 04)BbcD'Bbcia - 2c4D'BabBbc^c] + (d2 + mc4){ D'Bac[fvcib - fvbHc] + ' [(di - d2)^'bcBbcia

+ (mc4 - d2)BabQ'bcic + (2di - d2 - m€4)tt'abBbcic] 2

(4m (d - 3)C2 , m,\\'v\a ac[f bbc f ctb]

+ ( (d - 2) + mdVl abjfvH- fvH\

(d - 2) 1 ab

- 2m(d2 + mc4)e'\BabfB'

If we put

ci = -2c2, c3 = - —, di = d2 = -mc4 (A.3)

we obtain

-c2 f TA F'vab^acdHd - 2c4e'aB^abBbcic + 2m(c4 - 2c2)e'aBab

"( ^^ - mc) \Tc}DMc + (- "'^l'' j - f*]

- m c4 , , ,

(d - 2) V I ab

First two terms can be compensated by the following corrections to gauge transformations: sif'a - siB' ~ Babib

while the remaining terms require

4(d - 3)c2

c4 = 2c2, c4 = ———— ^ d = 4 (d - 2)

thus such solution indeed exists in d = 4 dimensions only.

nab transformations

With the same restrictions on parameters we get

{!Va\ ab cd f d A / o \i !v \ <~> ac bc n aba] F!v n fa - 4m(c4 - 2c2)\ab]Q! r B

- 2m(c4 - 2c2)e!aBabrjbc f! - m2(c - ^^ { ^ } f,arbc fvc

The first term can be compensated by the following correction

Sf! - rabf!b while the remaining ones again give

c4 = 2c2, d = 4

S transformations Similarly:

K-c4+1(d-r)| "O^D^a

+ 2,^.2 + c^vrv'' + B2

in agreement with all previous results.

A.3. Gravitational interaction

In this case we have to consider variations for all five transformations: rjab, Sa for graviton and rab, Sa, S for partially massless spin-2. It requires rather long calculations so we will not reproduce it here restricting ourselves with the main results.

Vertices with four derivatives

Using on-shell identities and field redefinitions can be written as follows

Li4=a0 j 'aavbacßj ^D^n^o^*+D^n^np**]

+ ai\ 'b \D'OvcdBacBbd

Vertex with three derivatives

As in the case of self-interaction all terms of the form DQBh and DoBf vanish on-shell or can be removed by field redefinitions. This leaves us with:

'2\ [bitt'abBcdOvcd + b2Ü'acBcdOvbd

+ b3nßcdBcdovab + b4tt'/dBabovcd]

Note that this structure is similar to one of 2-2-1 vertex with three derivatives that plays important role in the electromagnetic interactions for spin 2 particles [17].

Variations of order m require7:

U U t t 2m(d - 4)ao 4(d - 4)ao

= -4b1' b3 = b1' bl + b4 = - (d - 2) ' 01 = provided we introduce the following corrections to the gauge transformations:

B = b4Wabvab - ^^abnab] Thus at this stage we have two independent parameters a0 and say b4.

Vertices with two derivatives

The most general on-shell non-equivalent form looks like

L12={aa} [ci^^ad^vbdkac+C2ttl/bnvcdhac ]

+ { ITc} M/Vf + C4^iab^vCdfad + c&^f ]

+ e?a [C6B2h/ + C7BabBbchiC] (A.4)

Variations of order m2 require

C1 + C5 = -2mbi, C2 + C5 = m(b4 - bi)

C3 = —2c5, C4 = -C4, C7 = 4c6 -

(d - 2)

while corresponding corrections to the gauge transformations gave the form:

Sfia = -2c5(nabfib - oiabf) + ^ ci - md-T0) {nabhib - ^/blb)

Shia = 2c5{nabfib - ^iabib), SBi = 2c6B/fa (A.5)

Vertex with one derivative The most general ansatz is:

I [j ab r c n \ j o abi c Ti ] i j I I nab r c i c

Lii = ( ^ j [di^iabfvcBa + d2^iabhvcB^ + d3 j ^ \ Babfi/hvc Note that the only possible term without derivatives

l-iva\ f a fbi, c

f a f bh JfÂ fv ha

is forbidden by the invariance under the f transformations.

First of all note that solution with non-zero parameter c5 exists in d = 3 dimensions only. Recall that the Fradkin-Vasiliev formalism we use in the main part works in d > 4 dimensions only so it cannot reproduce such vertex. Note however that in the frame-like gauge invariant

7 We organize variations by the dimensionality of coefficients. E.g. variations of order m means coefficients of the form ma or b and so on.

formalism this vertex (having no more than two derivatives) has been constructed in [2o]. For the general d> 3 case we obtain two independent solutions with ao and b4 as free parameters:

m(d - 3)b4

c1 = -2mb1, c2 = m(b4 - b!), c6 = —-———

(d - 2)

c3 = c4 = c5 = d1 = d2 = d3 = o

Note at last that in d = 4 dimensions parameter ao is absent leaving us with one vertex only,

moreover, in this case all four derivative terms vanish on-shell.

References

[1] M.A. Vasiliev, Cubic interactions of bosonic higher spin gauge fields in AdS5, Nucl. Phys. B 616 (2oo1) 1o6-162, arXiv:hep-th/o1o62oo;

M.A. Vasiliev, Nucl. Phys. B 652 (2oo3) 4o7 (Erratum).

[2] K.B. Alkalaev, M.A. Vasiliev, N = 1 supersymmetric theory of higher spin gauge fields in AdS (5) at the cubic level, Nucl. Phys. B 655 (2oo3) 57-92, arXiv:hep-th/o2o6o68.

[3] N. Boulanger, S. Leclercq, Consistent couplings between spin-2 and spin-3 massless fields, JHEP o611 (2oo6) o34, arXiv:hep-th/o6o9221.

[4] N. Boulanger, S. Leclercq, P. Sundell, On the uniqueness of minimal coupling in higher-spin gauge theory, JHEP o8o8 (2oo8) o56, arXiv:o8o5.2764.

[5] Yu.M. Zinoviev, Spin 3 cubic vertices in a frame-like formalism, JHEP o8 (2o1o) o84, arXiv:1oo7.o158.

[6] R. Manvelyan, K. Mkrtchyan, W. Ruehl, General trilinear interaction for arbitrary even higher spin gauge fields, Nucl. Phys. B 836 (2o1o) 2o4, arXiv:1oo3.2877.

[7] R. Manvelyan, K. Mkrtchyan, W. Ruehl, A generating function for the cubic interactions of higher spin fields, Phys. Lett. B 696 (2o11) 41o, arXiv:1oo9.1o54.

[8] E. Joung, M. Taronna, Cubic interactions of massless higher spins in (A)dS: metric-like approach, Nucl. Phys. B 861 (2o12) 145, arXiv:111o.5918.

[9] G.L. Gomez, M. Henneaux, R. Rahman, Higher-spin fermionic gauge fields and their electromagnetic coupling, JHEP 12o8 (2o12) o93, arXiv:12o6.1o48.

[10] Marc Henneaux, Gustavo Lucena Gomez, Rakibur Rahman, Gravitational interactions of higher-spin fermions, JHEP 14o1 (2o14) o87, arXiv:131o.5152.

[11] R.R. Metsaev, Cubic interaction vertices of massive and massless higher spin fields, Nucl. Phys. B 759 (2oo6) 147, arXiv:hep-th/o512342.

[12] R.R. Metsaev, Cubic interaction vertices for fermionic and bosonic arbitrary spin fields, Nucl. Phys. B 859 (2o12) 13, arXiv:o712.3526.

[13] R.R. Metsaev, BRST-BV approach to cubic interaction vertices for massive and massless higher-spin fields, Phys. Lett. B 72o (2o13) 237, arXiv:12o5.3131.

[14] Yu.M. Zinoviev, On massive spin 2 interactions, Nucl. Phys. B 77o (2oo7) 83-1o6, arXiv:hep-th/o6o917o.

[15] R.R. Metsaev, Gravitational and higher-derivative interactions of massive spin 5/2 field in (A)dS space, Phys. Rev. D 77 (2oo8) o25o32, arXiv:hep-th/o612279.

[16] Yu.M. Zinoviev, On spin 3 interacting with gravity, Class. Quantum Gravity 26 (2oo9) o35o22, arXiv:o8o5.2226.

[17] Yu.M. Zinoviev, On massive spin 2 electromagnetic interactions, Nucl. Phys. B 821 (2oo9) 431-451, arXiv: o9o1.3462.

[18] A. Sagnotti, M. Taronna, String lessons for higher-spin interactions, Nucl. Phys. B 842 (2o11) 299, arXiv: 1oo6.5242.

[19] I.L. Buchbinder, T.V. Snegirev, Yu.M. Zinoviev, Cubic interaction vertex of higher-spin fields with external electromagnetic field, Nucl. Phys. B 864 (2o12) 694, arXiv:12o4.2341.

[20] Yu.M. Zinoviev, On massive gravity and bigravity in three dimensions, Class. Quantum Gravity 3o (2o13) o55oo5, arXiv:12o5.6892.

[21] I.L. Buchbinder, T.V. Snegirev, Yu.M. Zinoviev, On gravitational interactions for massive higher spins in AdS3, J. Phys. A 46 (2o13) 214o15, arXiv:12o8.o183.

[22] E. Joung, L. Lopez, M. Taronna, On the cubic interactions of massive and partially-massless higher spins in (A)dS, JHEP o7 (2o12) o41, arXiv:12o3.6578.

[23] Yu.M. Zinoviev, All spin-2 cubic vertices with two derivatives, Nucl. Phys. B 872 (2o13) 21, arXiv:13o2.1983.

[24] I.L. Buchbinder, P. Dempster, M. Tsulaia, Massive higher spin fields coupled to a scalar: aspects of interaction and causality, Nucl. Phys. B 877 (2o13) 26o, arXiv:13o8.5539.

[25] E.S. Fradkin, M.A. Vasiliev, On the gravitational interaction of massless higher-spin fields, Phys. Lett. B 189 (1987) 89.

[26] E.S. Fradkin, M.A. Vasiliev, Cubic interaction in extended theories of massless higher-spin fields, Nucl. Phys. B 291 (1987) 141.

[27] K.B. Alkalaev, FV-type action for AdS (5) mixed-symmetry fields, JHEP 11o3 (2o11) o31, arXiv:1o11.61o9.

[28] Nicolas Boulanger, E.D. Skvortsov, Yu.M. Zinoviev, Gravitational cubic interactions for a simple mixed-symmetry gauge field in AdS and flat backgrounds, J. Phys. A 44 (2o11) 4154o3, arXiv:11o7.1872.

[29] Nicolas Boulanger, E.D. Skvortsov, Higher-spin algebras and cubic interactions for simple mixed-symmetry fields in AdS spacetime, JHEP 11o9 (2o11) o63, arXiv:11o7.5o28.

[30] N. Boulanger, D. Ponomarev, E.D. Skvortsov, Non-abelian cubic vertices for higher-spin fields in anti-de Sitter space, JHEP 13o5 (2o13) oo8, arXiv:1211.6979.

[31] M.A. Vasiliev, 'Gauge' form of description of massless fields with arbitrary spin, Sov. J. Nucl. Phys. 32 (198o) 439.

[32] V.E. Lopatin, M.A. Vasiliev, Free massless bosonic fields of arbitrary spin in d-dimensional de Sitter space, Mod. Phys. Lett. A 3 (1988) 257.

[33] M.A. Vasiliev, Free massless fermionic fields of arbitrary spin in d-dimensional de Sitter space, Nucl. Phys. B 3o1 (1988) 26.

[34] M. Vasiliev, Cubic vertices for symmetric higher-spin gauge fields in (A)dSd, Nucl. Phys. B 862 (2o12) 341, arXiv: 11o8.5921.

[35] Yu.M. Zinoviev, Frame-like gauge invariant formulation for massive high spin particles, Nucl. Phys. B 8o8 (2oo9) 185, arXiv:o8o8.1778.

[36] Yu.M. Zinoviev, Towards frame-like gauge invariant formulation for massive mixed symmetry bosonic fields, Nucl. Phys. B 812 (2oo9) 46, arXiv:o8o9.3287.

[37] Yu.M. Zinoviev, Frame-like gauge invariant formulation for mixed symmetry fermionic fields, Nucl. Phys. B 821 (2oo9) 21-47, arXiv:o9o4.o549.

[38] Yu.M. Zinoviev, Towards frame-like gauge invariant formulation for massive mixed symmetry bosonic fields. II. General Young tableau with two rows, Nucl. Phys. B 826 (2o1o) 49o, arXiv:o9o7.214o.

[39] D.S. Ponomarev, M.A. Vasiliev, Frame-like action and unfolded formulation for massive higher-spin fields, Nucl. Phys. B 839 (2o1o) 466, arXiv:1oo1.oo62.

[40] Yu.M. Zinoviev, On electromagnetic interactions for massive mixed symmetry field, JHEP o3 (2o11) o82, arXiv: 1o12.27o6.

[41] Yu.M. Zinoviev, Gravitational cubic interactions for a massive mixed symmetry gauge field, Class. Quantum Gravity 29 (2o12) o15o13, arXiv:11o7.3222.

[42] S. Deser, A. Waldron, Gauge invariance and phases of massive higher spins in (A)dS, Phys. Rev. Lett. 87 (2oo1) o316o1, arXiv:hep-th/o1o2166.

[43] S. Deser, A. Waldron, Partial masslessness of higher spins in (A)dS, Nucl. Phys. B 6o7 (2oo1) 577, arXiv:hep-th/ o1o3198.

[44] S. Deser, A. Waldron, Null propagation of partially massless higher spins in (A)dS and cosmological constant speculations, Phys. Lett. B 513 (2oo1) 137, arXiv:hep-th/o1o5181.

[45] Yu.M. Zinoviev, On massive high spin particles in (A)dS, arXiv:hep-th/o1o8192.

[46] S. Deser, E. Joung, A. Waldron, Gravitational- and self-coupling of partially massless spin 2, Phys. Rev. D 86 (2o12) 1o4oo4, arXiv:13o1.4181.

[47] Claudia de Rham, Kurt Hinterbichler, Rachel A. Rosen, Andrew J. Tolley, Evidence for and obstructions to nonlinear partially massless gravity, Phys. Rev. D 88 (2o13) o24oo3, arXiv:13o2.oo25.