Supersymmetric 3-3-1 model
J. C. Montero, V. Pleitez, and M. C. Rodriguez
Instituto de Fı´sica Teo´rica, Universidade Estadual Paulista, Rua Pamplona, 145, 01405-900 Sa˜o Paulo, SP, Brazil
~Received 15 December 2000; published 10 January 2002!
We build a complete supersymmetric version of a 3-3-1 gauge model using the superfield formalism. We point out that a discrete symmetry, similar toRsymmetry in the minimal supersymmetric standard model, is possible to be defined in this model. Hence we have bothR-conserving andR-violating possibilities. Analysis of the mass spectrum of the neutral real scalar fields show that in this model the lightest scalar Higgs boson has a mass upper limit, and at the tree level it is 124.5 GeV for a given illustrative set of parameters.
DOI: 10.1103/PhysRevD.65.035006 PACS number~s!: 11.30.Pb, 12.60.Jv
I. INTRODUCTION
Although the standard model ~SM!, based on the gauge symmetry SU(3)c^SU(2)
L^U(1)Y, describes the
ob-served properties of charged leptons and quarks, it is not the ultimate theory. However, the necessity to go beyond it, from the experimental point of view, comes at the moment only from neutrino data @1#. If neutrinos are massive then new physics beyond the SM is needed. From the theoretical point of view, the SM cannot be a fundamental theory since it has so many parameters and some important questions such as that of the number of families do not have an answer in its context. On the other hand, it is not clear what the physics beyond the SM should be. An interesting possibility is that at the TeV scale physics would be described by models which share some of the flaws of the SM but give some insight concerning some questions which remain open in the SM context.
One of these possibilities is that, at energies of a few TeVs, the gauge symmetry may be SU(3)c^SU(3)
L ^U(1)N ~3-3-1 for shortness! instead of that of the SM
@2,3#. In fact, this may be the last symmetry involving the lightest elementary particles: leptons. The lepton sector is exactly the same as in the SM but now there is a symmetry, at large energies among, say e2, n
e, and e1. Once this
symmetry is imposed on the lightest generation and extended to the other leptonic generations it follows that the quark sector must be enlarged by considering exotic charged quarks. It means that some gauge bosons carry lepton and baryon quantum number. Although this model coincides at low energies with the SM it explains some fundamental questions that are accommodated, but not explained, in the SM. These questions are the following.
~i!The family number must be a multiple of three in order to cancel anomalies @2,3#. This result comes from the fact that the model is anomaly free only if we have equal number of triplets and antitriplets, counting the SU(3)c colors, and furthermore requiring the sum of all fermion charges to van-ish. However, each generation is anomalous, the anomaly cancellation occurs for the three, or multiple of three, to-gether and not generation by generation like in the SM. This may provide a first step towards answering the flavor ques-tion.
~ii! Why sin2uW,14 is observed. This point comes from the fact that in the model of Ref.@2#we have that theU(1)N
and SU(3)L coupling constants, g
8
andg, respectively, are related byt2[g
8
2
g2 5
sin2u
W
124 sin2u
W
. ~1!
Hence, this 3-3-1 model predicts that there exists an energy scale, saym, at which the model loses its perturbative char-acter. The value of m can be found through the condition sin2u
W(m)51/4. However, it is not clear at all what is the
value ofm; in fact, it has been argued that the upper limit on the vector bilepton masses is 3.5 TeV@4#instead of the 600 GeV given in Ref.@5#. Hence, if we want to implement su-persymmetry in this model, and to remain in a perturbative regime, it is natural that supersymmetry is broken at the TeV scale. This is very important because one of the motivations for supersymmetry is that it can help to understand the hier-archy problem: if it is broken at the TeV scale. Notwithstand-ing, in the context of the SM it is necessary to assume that the breakdown of supersymmetry happens at the TeV scale. However, other 3-3-1 models, i.e., with different representa-tion content, have a different upper limit for the maximal energy scale @6#.
~iii! The quantization of the electric charge is possible even in the SM context. This is because of the classical~ hy-percharge invariance of the Yukawa interactions! and quan-tum constraints ~anomalies! @7#. However, this occurs only family by family and if there are no right-handed neutrinos
~neutrinos if massive must be Majorana fields!; or, when the three families are considered together the quantization of the electric charge is possible only if right-handed neutrinos with Majorana mass term are introduced @8# or another Higgs doublet@9#or some neutral fermions@10#are introduced. On the other hand, in the 3-3-1 model @2,3,6#the charge quanti-zation in the three families case does not depend on if neu-trinos are massless or massive particles @11#.
ought to be also Majorana particles in order to retain both features of the electromagnetic interactions @8,12#. On the other hand, in all sorts of 3-3-1 models the quantization of the charge and the vectorial nature of the electromagnetic interactions are related one to another and are also indepen-dent of the nature of the neutrinos @13#.
Last but not least,~v!if we accept the criterion that par-ticle symmetries are determined by the known leptonic sec-tor, and if each generation is treated separately, thenSU(3)L
is the largest chiral symmetry group to be considered among (n,e,ec)L. The lepton family quantum number is gauged; only the total lepton number, L, remains a global quantum number~or equivalently we can defineF5B1L as the glo-bal conserved quantum number where B is the baryonic number @14#!. On the other hand, if right-handed neutrinos do exist, as it appears to be the case @1#, the symmetry among (ne,e,nec,ec)L would beSU(4)L^U(1)N @15#. This
is possibly the last symmetry among leptons. There is no room forSU(5)L^U(1)
Nif we restrict ourselves to the case
of leptons with electric charges 61,0 @16#. Hence, in this case all versions of the 3-3-1 model, for instance the one in Refs. @2,3,17#, and the one in Refs. @6,18,19#, are different SU(3)L-projections of the largerSU(4)L symmetry@15#.
Besides the characteristic features given above, which we can consider predictions of the model, the model has some interesting phenomenological consequences.~a!An extended version of some 3-3-1 models may solve the strong C P problem. It was shown by Pal @20# that in 3-3-1 models
@2,3,6,19# the more general Yukawa couplings admit a Peccei-Quinn symmetry @21#and that symmetry can be ex-tended to the Higgs potential and, therefore, making it a symmetry of the entire Lagrangian. This is obtained by in-troducing extra Higgs scalar multiplets transforming under the 3-3-1 symmetry as D;(1,10,23), for the model of Refs.@2,3#, orD;(1,10,21), for the model of Refs.@6,19#. In this case the resulting axion can be made invisible. The interesting thing is that in those sort of models the Peccei-Quinn symmetry is an automatic symmetry, in the sense that it does not have to be imposed separately on the Lagrangian but it is a consequence of the gauge symmetry and a discrete symmetry.~b!There exist new contributions to the neutrino-less double beta decay in models with three scalar triplets
@14# or in the model with the sextet @22#. If the model is extended with a neutral scalar singlet it is possible to have a safe Majoron-like Goldstone boson and there are also contri-butions to that decay with Majoron emission @22#. ~c!It is the simplest model that includes bileptons of both types: sca-lar and vector ones. In fact, although there are several models which include doubly charged scalar fields, not many of them incorporate doubly charged vector bosons: this is a par-ticularity of the 3-3-1 model of Refs. @2,3#. ~d! The model has several sources ofC Pviolation. In the 3-3-1 model@2,3#
we can implement the violation of the C P symmetry, spon-taneously @23,24# or explicitly @25#. In models with exotic leptons it is possible to implement softC Pviolation@26#.~e!
The extra neutral vector boson Z
8
conserves flavor in the leptonic but not in the quark sector. The couplings to the leptons are leptophobic because of the suppression factor (124sW2)1/2 but with some quarks there are enhancementsbecause of the factor (124sW2)21/2 @27#. ~f! Although the minimal scalar sector of the model is rather complicated, with at least three triplets, we would like to stress that it contains all extensions of the electroweak standard model with extra scalar fields: two or more doublets @28#, neutral gauge singlet @29#, or doubly charged scalar fields@30#, or a combination of all that. However, some couplings which are allowed in the multi-Higgs extensions are not in the present model when we consider an SU(2)^U(1) subgroup. In-versely, there are some interactions that are allowed in the present models that are not in the multi-Higgs extensions of the SM, for instance, trilinear couplings among the doublets which have no analog in the SM, or even in the minimal supersymmetric standard model ~MSSM!. It means that the model preserves the memory of the 3-3-1 original symmetry. Hence, in our opinion, the large Higgs sector is not an intrin-sic trouble of this model.~g!Even if we restrict ourselves to leptons of charge 0,61 we can have exotic neutral @18# or charged heavy leptons@17#.~h!Neutrinos can gain Majorana masses if we allow one of the neutral components of the scalar sextet to gain a nonzero vacuum expectation value
@31#, or if we introduce right-handed neutrinos@32#, or if we add either terms in the scalar potential that break the total lepton number or an extra charged lepton transforming as a singlet under the 3-3-1 symmetry@33#.
Of course, some of the benefits of this type of model, such as items~i!,~ii!, and~iv!above, can be considered only as a hint to the final resolution of those problems: they depend on the representation content and we can always ask ourselves what is the main principle behind the representation content. Anyway, we think that the 3-3-1 models have interesting features by themselves and that it is well motivated to gen-eralize them by introducing supersymmetry. In the present paper we built exhaustively the supersymmetric version of the 3-3-1 model of Refs.@2,3#. A first supersymmetric 3-3-1 model, without the introduction of the scalar sextet, was con-sidered some years ago by Duong and Ma @34#.
The outline of the paper is as follows. In Sec. II we present the representation content of the supersymmetric 3-3-1 model. We build the Lagrangian in Sec. III. In Sec. IV we analyze the scalar potential; in particular, we found the mass spectrum of the neutral scalar and have shown that the lightest scalar field has an upper limit of 124.5 GeV. Our conclusion and a comparison with the supersymmetric model of Ref. @34# are in the last section. In the Appendixes we show the scalar mass matrices and the constraint equations for completeness.
II. THE SUPERSYMMETRIC MODEL
The fact that in the 3-3-1 model of Refs.@2,3#we have the constraint at tree level sin2uW,1/4 means, as we said before,
Refs. @34,35#and we will comment on these later.
However, let us first consider the particle content of the model without supersymmetry @2,3#. We have the leptons transforming as
Ll5
S
nll
lc
D
L;~1,3,0!, l5e,m,t. ~2!
In parentheses it appears the transformation properties under the respective factors @SU(3)C,SU(3)L,U(1)N#. We have
not introduced right-handed neutrinos and for the moment we assume here that the neutrinos are massless; however, see
@31–33#.
In the quark sector, one quark family is also put in the triplet representation
Q1L5
S
u1d1
J
D
L;
S
3,3,23
D
, ~3!and the respective singlets are given by
u1cL;
S
3*,1,223
D
, d1L c ;S
3*,1,1 3
D
, JLc;
S
3*,1,25 3
D
,~4!
writing all the fields as left handed.
The other two quark generations we put in the antitriplet representation
Q2L5
S
d2u2
j1
D
L, Q3L5
S
d3u3
j2
D
L;
S
3,3*,213
D
, ~5!and also with the respective singlets,
u2L c ,
u3L
c ;
S
3*,1,22
3
D
, d2L c ,d3L
c ;
S
3*,1,13
D
,j1cL,jc2L;
S
3*,1,43
D
. ~6!On the other hand, the scalars which are necessary to generate the fermion masses are
h5
S
h0h12
h21
D
;~1,3,0!, r5
S
r1r0 r11
D
;~1,3,11!,
x5
S
x2 x22x0
D
;~1,3,21!, ~7!
and one way to obtain an arbitrary mass matrix for the lep-tons is to introduce the following symmetric antisextet:
S5
S
s10 h2 1
A
2 h12A
2h21
A
2H111 s2 0
A
2h12
A
2 s20A
2H222
D
;~1,6*,0!. ~8!
Now, we introduce the minimal set of particles in order to implement the supersymmetry @36#. We have the sleptons corresponding to the leptons in Eq.~2!, squarks related to the quarks in Eqs.~4!–~6!, and the Higgsinos related to the sca-lars given in Eqs. ~7! and ~8!. Besides, in order to cancel chiral anomalies generated by the superpartners of the sca-lars, we have to add the following Higgsinos in the respec-tive antimultiplets:
h ˜
8
5S
h ˜
8
0h ˜ 1
8
1 h ˜ 28
2D
L;~1,3*,0!, ˜r
8
5S
r ˜8
2r ˜
8
0r ˜
8
22D
L
;~1,3*,
21!,
x ˜
8
5S
x ˜
8
1x ˜
8
11x ˜
8
0D
L
;~1,3*,11!, ~9a!
S ˜
8
5S
s ˜ 1
8
0 h˜ 2
8
2A
2 h ˜ 18
1A
2h ˜ 2
8
2A
2 H ˜1
8
22 s˜28
0A
2h ˜ 1
8
1A
2 s ˜ 28
0A
2 H ˜2
8
11D
L;~1,6,0!. ~9b!
There are also the scalar partners of the Higgsinos defined in Eq.~9!and we will denote them byh
8
,r8
,x8
,S8
. This is the particle content which we will consider as the minimal 3-3-1s model if the charged lepton masses are generated by the antisextetS.Summarizing, we have in the 3-3-1s model the following superfields: Lˆe,m,t, Qˆ1,2,3, hˆ, rˆ, xˆ, Sˆ; hˆ
8
, rˆ8
, xˆ8
, Sˆ8
; uˆ1,2,3c , dˆ1,2,3c , Jˆc, andjˆ1,2c , i.e., 23 chiral superfields, and 17 vector superfields: Vˆa, Vˆa, and Vˆ8
. In the MSSM there are 14 chiral superfields and 12 vector superfields.III. THE LAGRANGIAN
With the superfields introduced in the last section we can build a supersymmetric invariant Lagrangian. It has the fol-lowing form:
L3315L
HereL
SUSY is the supersymmetric piece, whileLso f t
explic-itly breaks SUSY. Below we will write each of these Lagrangians in terms of the respective superfields.
A. The supersymmetric term
The supersymmetric term can be divided as follows:
LSUSY5LLe pton1LQuarks1LGauge1LScalar, ~11!
where each term is given by
L
Le pton5
E
d4u@L¯ˆ e2gV ˆLˆ#, ~12!
LQuarks5
E
d4u@Q¯ˆ1exp$@2g~Vˆc1Vˆ!1~2g8
/3!Vˆ8
#%Qˆ11Q¯ˆaexp$@2g~Vˆc1V¯ˆ!2~g
8
/3!Vˆ8
#%Qˆa1¯ˆuicexp$@2gV¯ˆc2~2g
8
/3!Vˆ8
#%uˆic1¯ˆdicexp$@2gV¯ˆc1~g
8
/3!Vˆ8
#%dˆic1¯ˆJcexp$@2gV¯ˆc2~5g
8
/3!Vˆ8
#%Jˆc1¯ˆjbcexp$@2gV¯ˆc1~4g
8
/3!Vˆ8
#%jˆbc# ~13!and
L
Gauge5
1 4
F
E
d2u@W
c aW
c a
1WaWa
1W
8
W8
#1
E
d2¯u@W¯ c aW¯c a
1W¯aW¯a1W¯
8
W¯8
#G
, ~14!where Vˆc5TaVˆac, V¯ˆc5T¯aVˆac, Vˆ5TaVˆa, V¯ˆ5T¯aVˆa, and Ta
5la/2 (¯Ta
52l*a/2) are the generators of triplets~ antitrip-lets!ofSU(3), i.e.,a51, . . . ,8, andgandg
8
are the gauge couplings of SU(3) and U(1), respectively. Wca, Wa, and W8
are the strength fields, and they are given byWaac52
1 8gD¯ D¯ e
22gVˆcD
ae2gV ˆ
c,
Waa52 1 8gD¯ D¯ e
22gVˆD ae2gV
ˆ
,
Wa
8
521
4D¯ D¯ DaVˆ
8
. ~15!Finally
LScalar5
E
d4u@h¯ˆ e2gVˆhˆ1¯ˆ er 2gVˆ1g8Vˆ8rˆ1x¯ˆ e2gVˆ2g8Vˆ8xˆ1¯ˆ eS 2gVˆSˆ1h¯ˆ
8
e2gVChˆ8
1¯ˆr8
e2gVC2g8Vˆ8rˆ8
1x¯ˆ
8
e2gV¯ˆ1g8Vˆ8xˆ8
1¯ˆS
8
e2gV¯ˆSˆ8
#1
E
d2uW1
E
d2¯ Wu¯ , ~16!whereWis the superpotential, which we discuss in the next subsection.
B. Superpotential
The superpotential of our model is given by
W5W2 2 1
W3
3 , ~17!
with W2 having only two chiral superfields and the terms permitted by our symmetry are
W25m0Lˆhˆ
8
1mhhˆhˆ8
1mrrˆrˆ8
1mxxˆxˆ8
1mSSˆSˆ8
,~18!
and in the case of three chiral superfields the terms are
W35l1eLˆLˆLˆ1l2eLˆLˆhˆ1l
3LˆLˆSˆ1l4eLˆxˆrˆ1f1erˆxˆhˆ
1f2hˆhˆ Sˆ1f3xˆrˆ Sˆ1f1
8
erˆ8
xˆ8
hˆ8
1f28
hˆ8
hˆ8
Sˆ8
1f3
8
xˆ8
rˆ8
Sˆ8
1(
i@k1iQˆ1hˆ
8
uˆic1k2iQˆ1rˆ8
dˆic#1k3Qˆ1xˆ
8
Jˆc1(
ai
@k4aiQˆahˆ dˆi c
1k5aiQˆarˆ uˆi c#
1
(
ab k6abQ
ˆaxˆ jˆbc
1
(
ai j
k7ai jQˆaLˆidˆjc
1
(
i,j,k j1i jkdˆi c
dˆcjuˆkc1
(
i jb j2i jbuˆi c
uˆjcjˆbc1
(
ib j3ibdˆic Jˆcjˆbc,
~19!
withi,j,k51,2,3, a52,3, andb51,2.
All the seven neutral scalar components h0,r0,x0,s
2 0,h
8
0,r8
0, andx8
0 gain nonzero vacuum expec-tation values. This arises from the mass matrices for quarks. In fact, defining^
h0&
5vh/
A
2,^
h08
&
5vh8
/A
2, etc, from the superpotential in Eq.~19!the following mass matrices arise:Gu
5 1
A
2S
k11vh
8
k12vh8
k13vh8
k521vr k522vr k523vr k531vr k532vr k533vrD
, ~20!
Gd
5 1
A
2S
k21vr
8
k22vr
8
k23vr
8
k421vh k422vh k423vh k431vh k432vh k4333vh
D
, ~21!
for the d quarks, and for the exotic quarks, J and j1,2, we have MJ5k3vx
8
andGj5 vx
A
2S
k621 k622
k631 k632
D
, ~22! respectively.From Eqs.~20!,~21!, and~22!we see that all the vacuum expectation values~VEVs!have to be different from zero in order to give mass to all quarks. Notice also that the u-like and d-like mass matrices have no common VEVs. On the other hand, the charged lepton mass matrix is already given by Mi jl5vs
2l3i j/
A
2, where vs2 is the VEV of the^
s2 0&
component of the antisextetSin Eq.~8!. However,vs1,2
8
can both be zero since the sextetS8
does not couple to leptons at all.The terms which are proportional to the following con-stants: m0 in Eq.~18! andl1, l4, f2, f2
8
, k7, andj1,2,3 in Eq. ~19! violate the conservation of the F5B1L quantumnumber. For instance, if we allow the j1 term it implies in proton decay@35#. However, if we assume the globalU(1)F
symmetry, it allows us to introduce the R-conserving sym-metry @37#, defined asR5(21)3F12S. The Fnumber
attri-bution is
F~U22!
5F~V2!
52F~J1!5F~J2,3!5F~r22!
5F~x22!
5F~x2! 5F~h
2 2!
5F~s 1 0!
52,
~23!
withF50 for the other Higgs scalar, while for leptons and the known quarks F coincides with the total lepton and baryon numbers, respectively. As in the MSSM this defini-tion implies that all known standard model’s particles have even Rparity while their supersymmetric partners have odd R parity. The termsj2,l4 were not considered in Ref.@35#. However, the term withj2 involves an exotic quark~heavier than the proton!so the analysis in that reference is still valid. As usual, the supersymmetry breaking is accomplished by including the most general renormalizable soft-supersymmetry breaking terms but now, they must be also consistent with the 3-3-1 gauge symmetry. We will also in-clude terms which explicitly violate the R-like symmetry. These soft terms are given by
L
so f t52
1
2
F
mlc(
a lcal c a
1ml
(
a~ lal
a!1m
8
ll1H.c.G
2mL2L˜†˜L2mQ21Q˜1†Q˜11(
i
@˜uic†mu
i
2˜u
i c
2˜dic†md
i
2d˜
i c#
2mJ2˜Jc†˜Jc2
(
b j
˜bc†m
jb
2˜j
b c
2
(
a mQa
2 Q˜
a
†Q˜
a2mh2h†h2mx2x†x2m2rr†r2ms2Tr~S†S!2mh8
2 h
8
†h8
2mr 8
2 r
8
†r8
2mx 82 x
8
†x8
2ms 82
Tr~S
8
†S8
!2F
k1erxh1k2hhS†1k3xrS†1k8
1er8
x8
h8
1k28
h8
h8
S8
†1k38
x8
r8
S8
† 1M2L˜h†1«0
(
i jk ei jkL ˜
iL˜jL˜k1«1
(
i jk ei jkL ˜
iL˜jhk1«2
(
i j L ˜
iL˜jSi j1«3
(
i jk ei jkL ˜
ixjrk
1
(
i Q ˜
1~z1ih
8
˜uic1z2ir8
˜dic1z3Jx8
˜Jc!1(
a Q˜a
F
(
iS
v1aih˜dic1v2airu˜ic1
(
j v3ai jL ˜
i˜djc
D
1(
b v4abxj
˜
b c
G
1
(
i
S
(
jk§1i jk˜dic˜djc˜ukc1
(
a
F
§2iad˜ic˜Jc˜jac1
(
j§3i ja˜uic˜ucj˜jac
GD
1H.c.G
. ~24!The terms proportional to k2, k2
8
, M2,«0, «3, v3, and§1,2,3 violates theR-parity symmetry. The SU(3) invariance tell us that
mL5
S
m˜n 0 0
0 ml˜ 0 0 0 ml˜c
D
, ~25!
and we need ml˜c5ml˜5mn˜ and the same for the other mass
parameters. More details of the Lagrangian are given else-where@38#.
IV. THE SCALAR POTENTIAL
The scalar potential is written as
V3315VD1VF1Vsoft, ~26a!
VD52LD5
1 2~D
aDa
1DD!g
8
2
2 ~r †r
2r
8
†r8
2x†x1x8
†x8
!2 1g2
8
(
i,j ~hi†l
i j ah
j1ri
†l
i j ar
j1xi
†l
i j ax
j
1Si j†lajkSkl2hi
8
†li j*ahj8
2ri8
†li j*arj8
2xi8
†li j*ax8
j2Si j8
†ljk*aSkl8
!2, ~26b!VF52LF5
(
m Fm*Fm5
(
i,j,kF
U
mh 2 hi
8
1f1
3 ei jkrjxk1 2f2
3 hiSi j
U
21
U
mr 2 ri8
1f1
3 ei jkxjhk1 f3 3 xiSi j
U
2
1
U
mx 2 xi8
1f1
3 ei jkrjhk1 f3
3 riSi j
U
21
U
ms 2 Si j8
1f2 3 hihj1
f3 3 xirj
U
2
1
U
mh 2 hi1f1
8
3 ei jkr
8
jxk8
12f2
8
3 hi8
Si j8
U
2
1
U
mr 2 ri1 f1
8
3 ei jkx
8
jhk8
1 f38
3 xi
8
Si j8
U
21
U
mx 2 xi1f1
8
3 ei jkr
8
jhk8
1 f38
3 ri
8
Si j8
U
21
U
ms 2 Si j1f2
8
3 hi
8
h8
j1 f38
3 xi
8
rj8
U
2G
, ~26c!Vso f t52Lso f t
scalar
5mh2h†h
1mr2r†r1mx2x†x1ms
2Tr~
S†S!1mh 8
2 h
8
†h8
1mr8
2 r
8
†r8
1mx 8
2 x
8
†x8
1ms 8
2
Tr~S
8
†S8
!1@k1e rxh1k2hS†h1k3xTS†r1k1
8
e r8
x8
h8
1k28
h8
S8
†h8
1k38
x8
TS8
†r8
1H.c.#. ~26d!Note that k1,2,3,k1,2,3
8
has dimension of mass and that the terms which are proportional to k2,k28
and f2,f28
violate the Rparity.It is instructive to rewrite Eqs. ~26b!as follows:
VD5g
8
22 ~r †r
2x†x2r
8
†r8
1x8
†x8
!21g 28
F
4 3(
i~Xi†Xi!2
12
(
i,j ~Xi
† Xj!~Xj
†
Xi!12
(
i ~Xi†
S!~S†Xi!
24 3
(
i,j~Xi†Xi!~Xj
† Xj!2
2 3Tr~S
†S!
(
i
~Xi†Xi!
12 Tr@~S†S!2#22 3~TrS
†S!2
1pt
G
, ~27!where ‘‘pt’’ in the expression above denotes the replacements Xi
8
↔Xibut not ing
8
which is always the coupling constantof theU(1)Nfactor. In the same way we rewrite Eq.~26c!as
VF5
(
i
mX
i
2
4 ~Xi†Xi1pt!1
umS2u 4 @Tr~S
†S!
1pt#116
(
iÞjÞk
H
mX
i
*
6 @f1ei jkXi
8
†XjXk1f18
ei jkXi†X8
jXk8
#1f32
F
mh*h8
†Sh1mS*
2 h †S
8
hG
1pt1f63@mr*r8
†Sx1mx*x
8
†Sr1m*Sx†S8
r#1pt1H.c.J
1uf1u2
F
(
iÞj
~Xi†Xi!~Xj
†
Xj!2~Xj
† Xi!~Xi
†
Xj!
G
1pt14uf2u2 9 @~hS!
†~hS!
1~h†h!2#
1pt1uf3u 2
9 @~xS! †~xS!
1~rS!†~rS!1~x†x!†~r†r!# 1pt1
2f1*f2 9 e~rx!
†hS 1pt
1
F
f1*f3 9 e~xh!
†xS1pt1f2*f3 9 ~h
†x!~h†r!
1pt1H.c.
G
, ~28!where ‘‘pt’’ in the expression above denotes as before the replacementsXi
8
↔Xi, andf1,2,3
8
↔f1,2,3, andk1,2,38
↔k1,2,3. We have omitted SU(3) indices since we have denoted the unprimed triplets wherever it is possible as Xi5h,r,x and Xi8
We can now work out the mass spectra of the scalar and pseudoscalar fields by making a shift of the form X →(1/
A
2)(vX1HX1iFX) ~similarly for the case of the primed fields!for all the neutral scalar fields of the multiplets Xi. Note thatHX andFX are not mass eigenstates yet. We will denote Hi,i51, . . . ,8 and Ai,i51, . . . ,6 therespec-tive massive fields; G1,2 will denote the two neutral Gold-stone bosons. The mass matrices appear in the Appendix A, for the real scalars, and in the Appendix B for the pseudo-scalar case. The constraint equations are given in the Appen-dix C. We will use the following set of parameters in the scalar potential below:
f15f351, f1
8
5f8
351026 ~dimensionless!, ~29!and
2k15k1
8
510, k35k38
52100,2mh5mr52ms5mx51000 ~in GeV!, ~30!
we also use the constraintVh21Vr212V225(246 GeV)2 com-ing from MW, where, we have defined Vh25v2h1vh
8
2, Vr2 5vr21vr8
2, and V225vs2 2
1v
s28
2
. Assuming that vh520, vx 51000, vs
2510, and vh
8
5vr8
5vs8
25vx
8
51 in GeV, the value ofvr is fixed by the constraint above.With this set of values for the parameters the real mass eigenstates Hi are obtained by the diagonalization of the mass matrix given in the Appendix A. Besides the constraint equations ~Appendix C! and imposing the positivity of the eigenvalues~mass square!, and the values for the parameters given above, we obtain the following values for the masses of the scalar sector ~in GeV!: MHi5121.01,
277.14,515.26,963.68,1218.8,1243.24,3797.86, and 4516.43, wherei51, . . . ,8 andMHj.MHi withj.i. In the
pseudo-scalar sector we have verified analytically that the mass ma-trix in the Appendix B, has two Goldstone bosons as it should be. The other six physical pseudoscalars have the following masses, with the same parameters as before, in GeV, MAi5276.4,515.3,963.65,1243.24,3797.85, and
4516.43.
The behavior of the lightest scalar (H1) and pseudoscalar (A1) as a function ofvxis shown in Fig. 1 for a given choice of the parameters, we see that, at the tree level, there is an upper limit for the mass of the lightest scalar MH1,124.5
GeV and that for these values of the parameters MA1
.MZ. Other values of the parameters give higher or lower
values for the upper limit of MH1. Of course, radiative
cor-rections have to be taken into account, however, this has to be done in the context of the supersymmetric 3-3-1 model which is not in the scope of the present work. Hence the mass square of the lightest real scalar boson has an upper bound ~see Fig. 1!
MH
1 2 <~
124.51e!2 GeV2, ~31!
where 124.5 GeV is the tree value (e50). We recall that in the MSSM if MA1.MZ the upper limit on the mass of the
lightest neutral scalar is MZ at the tree level but radiative
corrections raise it to 130 GeV @39#.
V. CONCLUSIONS
We have built the complete supersymmetric version of the 3-3-1 model of Refs.@2,3#. Another possibility in this 3-3-1 model which avoids the introduction of the scalar sextet,S, was considered some years ago by Duong and Ma, Ref.@34#, who built the supersymmetric version of that model. The sextet was substituted by a single charged lepton singlet EL
;(1,1) andELc;(1,21). Here we would like to point out the differences between our version of the supersymmetric 3-3-1 model and that of Ref. @34#. ~a! Duong and Ma as-sumed that the breaking of SU(3)L^U(1)N→SU(2)L ^U(1)
Yoccurred before the breaking of supersymmetry and
the resulting model is a supersymmetric SU(2)L^U(1)Y
model. Even in this case the scalar potential involving dou-blets of the residual gauge symmetry does not coincide with the potential of the MSSM. In the present work, we have considered that the supersymmetry is broken at the same time as the 3-3-1 gauge symmetry. Hence, we have to con-sider the complete 3-3-1 scalar potential. It means that in the Duong and Ma supersymmetric model there are no doubly charged charginos and exotic charged squarks. ~b! In Ref.
@34#it was assumed that some of the VEVs have zero value, unlikely we have considered all ~but s2
8
0 and s10) of them different from zero. Hence we are able to obtain realistic quark and charged lepton masses, as can be seen from Eqs.~20!,~21!, and~22!. In Ref.@34#some of these masses have to be generated by radiative corrections @40#. From ~a! and
~b!we see that the supersymmetric 3-3-1 model considered in this work has different phenomenological features from the supersymmetric 3-3-1 model of Duong and Ma.
On the other hand, we would like to recall that in the MSSM with soft-breaking terms, it has been shown that at the tree level the lightest scalar has a mass which is less than MZ if the mass of the top quark has an upper bound of 200
FIG. 1. The eigenvalues of the mass matrix given in Appendix A; MH1 is the mass of the lightest scalar andMAthe mass of the
GeV@41# and this upper limit does not depend on the scale of supersymmetry masses and on the scale of supersymmetry breaking and holds independently of the short distance or large mass behavior of the theory@42#and it does not depend on the number of the Higgs doublets@43#. Radiative correc-tions@42#and the addition of extra Higgs multiplets@42,44#
shift the limit above depending on the top mass or on the type of extra scalars. However, in the 3-3-1s that we have built here the limit of Ref.@41#is avoided.
From the phenomenological point of view there are sev-eral possibilities. Since it is possible to define the R-parity symmetry, the phenomenology of this model with R parity conserved has similar features to that of the R-conserving MSSM: the supersymmetric particles are pair produced and the lightest neutralino is the lightest supersymmetric particle. The mass spectra of all particles in this model are considered in Ref. @38#. However, there are differences between this model and the MSSM with or withoutR-parity breaking: due to the fact that there are doubly charged scalar and vector fields. Hence, we have doubly charged charginos which are mixtures of the superpartners of theU-vector boson with the doubly charged Higgsinos. This implies new interactions that are not present in the MSSM, for instance x˜22˜x0U11, x
˜2x˜2U11, l˜2l2x˜11, where x˜11 denotes any doubly charged chargino. Moreover, in the chargino production, be-sides the usual mechanism, we have additional contributions coming from theU-bilepton in theschannel. Due to this fact we expect that there will be an enhancement in the cross section of production of these particles in e2e2 colliders, such as the Next Linear Collider ~NLC! @38#. We will also have the singly charged charginos and neutralinos, as in the MSSM, where there are processes like l˜2l1x˜0, n˜
ll2˜x1,
with l˜ denoting any slepton; ˜x2 denotes singly charged chargino and˜nL denotes any sneutrino. The only difference is that in the MSSM there are five neutralinos and in the 3-3-1s model there are eight neutralinos.
Finally, we would like to call attention that, whatever the energy scalem at which sin2u
W(m)51/4 is in the
nonsuper-symmetric 3-3-1 model, when supersymmetry is added it will result in a rather different value form. In conclusion, we can say that the present model has a rich phenomenology that deserves to be studied in more detail.
ACKNOWLEDGMENTS
This work was supported by Fundac¸a˜o de Amparo a` Pes-quisa do Estado de Sa˜o Paulo~FAPESP!, Conselho Nacional de Cieˆncia e Tecnologia~CNPq!and by Programa de Apoio a Nu´cleos de Exceleˆncia ~PRONEX!. One of us ~M.C.R.!
would like to thank the Laboratoire de Physique Mathe´ma-tique et The´orique, Universite´ Montpellier II, for its kind hospitality and also M. Capdequi-Peyrane`re and G. Moultaka for useful discussions.
APPENDIX A: MASS MATRIX OF THE SCALAR NEUTRAL FIELDS
Here we write down the complete symmetric mass matrix in the scalarC P-even sector; the constraint equations given
in the Appendix C have been already taken into account:
M115
g2vh2
3 1
1 18
A
2vh~f1f3vr2vs
2218k1vrvx13f1vr
8
mrvx1f1f3vs
2vx 2
23f1
8
mhvr8
vx8
13f1mxvrvx8
!,M1252
g2vhvr
6 1
1
9
A
2S
A
2f1 2vhvr2f1f3vrvs
2
19k1vx2 3 2mxvx
8
D
,M1352g
2v
hvr
6 1
1 9
A
2S
9k1vr2 3 2f1mrvr
8
1
A
2f12vhvx2f1f3vs2vx
D
,M145 g2vhvs
2
6 2
f1f3
18
A
2~vr21vx2!, M1552 g2vhvh
8
3 ,
M165
g2vhv
r
8
6 2
1 6
A
2~mrvx2mhv
x
8
!,M175
g2vhvx
8
6 1
1 6
A
2~f18
mhvr
8
2f1mxvr!,M185
g2vhvs
2
6 ,
M225
S
g2 3 1g
8
2
D
vr
2 2
vx 12
A
2vr~12k1vh16
A
2k3vs2
12f1mhvh
8
1A
2f3msvs2
8
!1 vx
8
12
A
2vr~2f1
8
mrvh8
2
A
2f38
mrvs2
8
12f1mxvh2A
2mxvs2vx
8
!,M2352
S
g2 6 1g
8
2
D
vrvx1 1 12
A
2~12k1vh16
A
2k3vs2
12f
8
mhvh8
1A
2f3msvs2
8
!1 vrvx9 ~f1 2
1f32!,
M245
g2 12vrvx1
1
18
A
2S
22f1f3vhvr1
A
2f 3 2vs2vr
19
A
2k3vx1 3A
2f3mx vx
8
D
,M255
g2 6 vh
8
vr11 6
A
2~f1mhvx2f 1
8
mrvM2652
S
g2 3 1g
8
2
D
vrvr8
3 ,M275
S
g2 6 1g
8
2
D
vrvx
8
2 mr12
A
2~2f18
vh
8
2f38
vs2
8
!2 mx 12
A
2~2f1vh2f3vs
2!,
M2852
g2vrvs
2
8
12 1
1
12~f3msvx1f3
8
mrvx8
!,M335
S
g 23 1g
8
2D
vx
2
2 1
12
A
2vxS
12k1vhvr1 12
A
2k3 vrvs2
12f1mhv
8
hvr22f1mrvhvr8
1A
2f3mrvr8
vs2
1
A
2f3msvrvs2
8
22f18
mxvh8
v8
r1A
2f3mxvr8
vs2
8
D
,M345
g2
12vs2vx1 1 18
A
2S
9
A
2k3 vr13
A
2f3mr vr8
22f1f3vhvx1
A
2f32vs2vx
D
,M355g 2
6 vh
8
vx1 1 6A
2~f1mrvr2f 1
8
mxvr8
!,M365
S
g2 6 1g
8
2
D
vr
8
vx11
12
A
2~22f1mrvh1
A
2f3mrvs2
22f1
8
mxvh8
1A
2f 38
mxvs2
8
!,M3752
S
g 23 1g
8
2D
vxvx
8
,M3852
g2
12vs
8
2vx1 112~f3msvr1f3
8
mxvr8
!,M445g 2
12vs2 2
1 1
18
A
2vs2
S
f1f3vhvr22 18
A
2k3 vrvx2 3
A
2f3mrvr
8
vx1f1f3vhvr21 3A
2f38
ms vr8
vx8
2 3
A
2f3mx vrvx8
D
,M455
g2 6 vh
8
vs2,M4652
g2
12vr
8
vs21 112~f3mrvx1f3
8
msvx8
!,M4752
g2
12vs2vx
8
1 112~f3
8
msv8
r1f3mxvr!,M4852g
2
12vs2vs
8
2,M555
g2 3 vh
8
2
1 1
18
A
2vh8
~f1
8
f38
vr8
2vs2
8
23f1mrvrvh13f1
8
mxvr8
vx218k18
vr8
vx8
13f18
mrvrvx8
1f1
8
f3vs2
8
vx8
2!,M5652
g2 6 vh
8
vr8
11
9
A
2S
A
2f18
2vh
8
vr8
2f 18
f38
vr8
vs2
8
23
2f1
8
mxvx19k 18
vx8
D
,M5752
g2 6 vh
8
vx8
11 9
A
2S
9k18
v
r
8
232f1
8
mrvr1A
2f18
2vh
8
vx
8
2f1
8
f38
vs2vx
8
D
,M5852g
2
6 vh
8
vs8
22f1
8
f38
18
A
2~vr
8
21vx8
2!,M665
S
g 23 1g
8
2D
vr
8
21 112
A
2vr8
S
2f1mrvhvx
2
A
2f3mrvs2vx12f1
8
mxvh8
vx2A
2f38
mxvs8
2vx212k1
8
vh8
vx8
2 12A
2k38
vs2
8
vx8
22f 18
mhvhvx8
2
A
2f38
msvs2vx
8
D
,M6752
S
g2 6 1g
8
2
D
vr
8
vx8
11
12
A
2S
12k18
vh8
112
A
2k38
vs2
8
12f1
8
mhvh1A
2f38
msvs21 3
A
2f18
2vr
8
vx8
1 3
A
2f38
2vr
8
vx8
D
,M685
g2
12vr
8
vs8
21f3
8
vr
8
18
A
2~A
2f38
vs2
M775
S
g2 3 1g
8
2
D
vx
8
22 112
A
2vx8
~12k1
8
vh8
vr
8
112k38
vr
8
vs2
8
12f1
8
mhvhvr8
22f18
mrvh8
vr1A
2f38
mrvrvs2
1
A
2f38
msvr
8
vs222f1mxvhvr1
A
2f3mxvrvs2!,M785
g2
12vs
8
2vx8
1 112~6k3
8
vr8
1f38
mrvr!1 f3
8
vx8
18A
2~f38
vs
2
8
2f18
vh8
!,M885
g2 12vs
8
2221 18
A
2vs2
8
S
f18
f38
vh
8
vr
8
21 3
A
2f3ms vrvx1 3
A
2f38
mx vr8
vx118
A
2k38
vrvx8
13
A
2f38
mx vr8
vx1 18
A
2k38
vr8
vx8
13
A
2f38
mrvrvx
8
2f18
f38
vh8
vx8
2D
.This mass matrix has no Goldstone bosons and eight mass eigenstates. Some typical values of the masses of these sca-lars, for a set of values of the parameters, are given in the text. In Fig. 1 we show the behavior of the mass of the lightest scalarH1with thevx, the largest VEV in the model.
APPENDIX B: MASS MATRIX OF THE PSEUDOSCALAR NEUTRAL FIELDS
The complete symmetric mass matrix in theC P-odd sca-lar sector, with the constraint equations of Appendix C taken into account, is given by
M115 1
18
A
2vh~f1f3v
r
2 vs
2218k1vrvx13f1mrvr
8
vx8
!,M125 1
6
A
2~f1mx26f1 vx!,M135 1
6
A
2~f1mrvr
8
26k1vr!,M145 f1f3
18
A
2~vr21vx2!,
M1550,
M165 1
6
A
2~f1mh vx
8
2f18
mrvx!,M175 1
6
A
2~f18
mhvr
8
2f1mxvr!, M1850,M225 1
6
A
2vrS
26k1vhvx2 6
A
2k3 vs2vx2f1mhvh
8
vx2 1
A
2f3ms vs2
8
vx1f1
8
mrvh8
vx
8
2 1A
2f38
mr vs2
8
vx
8
1f1mxvhvx
8
2 1A
2f3mx vs2vx
8
D
,M235 1
6
A
2S
26k1 vh26
A
2k3 vs2
2f1mhvh
8
2 1A
2ms vs2
8
D
,M2451
12~6k3vx1f3mxvx
8
!,M255 1
6
A
2~f1mh vx2f1
8
mrvx8
!, M2650,M275 1
12
A
2~22f18
mrvh
8
1A
2f 38
mrvs2
8
22f1mxvh1
A
2f3mxvs2!,
M285 1
12~f3msvx1f3
8
mrvx8
!,M335 1
6
A
2vxS
26f1k1vhvr2 6
A
2k3 vrvs22f1mhvh
8
vr1f1mrvhv
r
8
2 1A
2f3mr vr
8
vs22 1
A
2f3ms vrvs2
8
1f1
8
mxvh8
vr
8
2 1A
2f38
mx vr
8
vs2
8
D
,M3451
12~6k3vr1f3mrvr
8
!,M355 1
A
2~f1mh vr2f1
8
mxvx
8
!,M365 1
12
A
2~22f1mrvh1
A
2f 3mrvs2
22f1
8
mxvh8
1A
2f 38
mxvs2
8
!,M3750, M3851
M445 1
18
A
2vs2
S
f1f3vhv
r
2 2 18
A
2k3 vrvx23
A
2mr vr
8
vx118
A
2k3 vrvx23
A
2f3mrvr
8
vx1f1f3vhvx22 3
A
2f38
ms vr8
vx8
23
A
2f3mx vrvx8
D
,M4550, M4652 1
12~f3mrvx1f3
8
msvx8
!,M4752 1
12~f3
8
mrvr8
1f3mxvr8
!, M4850,M555 1
18
A
2vh8
~f1
8
f38
vr
8
2vs2
8
23f1mhvrvx13f 18
mxvr
8
vx218k1
8
vr8
vx8
13f 18
mrvrvx8
1f 18
f38
vs2
8
vx8
213f1
8
mrvrvx8
1f18
f38
vs2
8
vx8
2!,M565 f1f3
18
A
2~mx vx2k1
8
vx
8
!,M575 1
6
A
2~26k18
vr
8
1f18
mrvr!,M585 f1
8
f38
18
A
2~vr
8
22vx8
2!,M665 1
12
A
2vr8
S
2f1mrvhvx2
A
2f3mrvs2vx
12f1
8
mxvh8
vx2A
2f 38
mxvs2
8
vx212k 18
vh8
vx
8
2 12
A
2k38
vs2
8
vx8
22f 18
mhvhvx8
2A
2msvs2vx
8
D
,M675 1
12
A
2S
212k18
vh8
212
A
2k38
vs2
8
22f18
mhvh2
A
2f38
msvs2
D
,M6851
12~2f3
8
mxvx16k38
vx8
!,M775 1
12
A
2vx8
S
212k3
8
vh8
vr
8
2 12A
2k38
vr
8
vs2
8
22f1
8
mhvhvr
8
12f18
mrvh8
vr2A
2f 38
mrvrvs2
8
D
,M785 1
12~6k3
8
vr8
2f38
mrvr!,M885 1
18
A
2vs2
8
S
f18
f38
vh
8
vr
8
22 3
A
2ms vrvx23
A
2mx vr
8
vx2 18
A
2k38
vr8
vx8
23
A
2f38
mr vrvx8
1f1
8
f38
vh8
vx8
2D
.This mass matrix has two Goldstone bosons and six mass eigenstates. In Fig. 1 we show the behavior of the mass of the lightest pseudoscalar scalarA1as a function ofvx. Typi-cal values for the masses in this sector for a set of values of the parameters are given in the text.
APPENDIX C: CONSTRAINT EQUATIONS
The constraint equations are
th vh5
g2 12~2vh
2
22vh
8
22v2r1vr8
22vs2 2
1vs
2
8
22vx21vx
8
2!1mh211 4mh
2 1 f1
2
18~vr 2
1vx2!1 f1f3
18
A
2 vs2
vh ~ vr21vx2!
1k1
A
2 vrvxvh 1
1 6
A
2vh~f1mrvr
8
vx1f1mxvrvx8
1f1
8
mhvr8
vx8
!,tr
vr5
g2 12
S
2vh2
1vh
8
212vr
2 22v
r
8
2112v
s2
2 212v
s2
8
22v
x
2
1vx
8
2D
1 g8
22 ~vr 2
2vr
8
22vx21vx8
2!1 f12 18~vh2 1vx2!
1 f3 2
36~vs2 2
12vx2!2 f1f3
9
A
2 vhvs21mr 2
11 4mr
2
1 k1
A
2 vhvxvr 1
k3 2
vs
2vx
vr 1
f1
6
A
2vr~mhvh
8
vx1mxvhvx8
!1 f3 12vr~ms
vs
2
8
vx1mxvs2vx
8
!1f3
8
12vrmr vs
2