Scholarly article on topic 'Higgs self-coupling in the MSSM and NMSSM after the LHC Run 1'

Higgs self-coupling in the MSSM and NMSSM after the LHC Run 1 Academic research paper on "Physical sciences"

CC BY
0
0
Share paper
Academic journal
Physics Letters B
OECD Field of science
Keywords
{}

Abstract of research paper on Physical sciences, author of scientific article — Lei Wu, Jin Min Yang, C.-P. Yuan, Mengchao Zhang

Abstract Measuring the Higgs self-coupling is one of the crucial physics goals at the LHC Run-2 and other future colliders. In this work, we attempt to figure out the size of SUSY effects on the trilinear self-coupling of the 125 GeV Higgs boson in the MSSM and NMSSM after the LHC Run-1. Taking account of current experimental constraints, such as the Higgs data, flavor constraints, electroweak precision observables and dark matter detections, we obtain the observations: (1) In the MSSM, the ratio λ 3 h MSSM / λ 3 h SM has been tightly constrained by the LHC data, which can be only slightly smaller than 1 and minimally reach 97%; (2) In the NMSSM with λ < 0.7 , a sizable reduction of λ 3 h 2 NMSSM / λ 3 h 2 SM can occur and minimally reach 10% when the lightest CP-even Higgs boson mass m h 1 is close to the SM-like Higgs boson m h 2 due to the large mixing angle between the singlet and doublet Higgs bosons; (3) In the NMSSM with λ > 0.7 , a large enhancement or reduction − 1.1 < λ 3 h 1 NMSSM / λ 3 h 1 SM < 2 can occur, which is accompanied by a sizable change of h 1 τ + τ − coupling. The future colliders, such as the HL-LHC and ILC, will have the capacity to test these large deviations in the NMSSM.

Academic research paper on topic "Higgs self-coupling in the MSSM and NMSSM after the LHC Run 1"

Contents lists available at ScienceDirect

Physics Letters B

www.elsevier.com/locate/physletb

Higgs self-coupling in the MSSM and NMSSM after the LHC Run 1

Lei Wua *, Jin Min Yangb, C.-P. Yuanc, Mengchao Zhangb*

a AfiC Centre of Excellence for Particle Physics at the Terascale, School of Physics, The University of Sydney, NSW2006, Australia b State Key Laboratory of Theoretical Physics, Institute of Theoretical Physics, Academia Sinica, Beijing 100190, China c Department of Physics and Astronomy, Michigan State University, East Lansing, MI 48824, USA

CrossMark

A R T I C L E I N F 0

Article history:

Received 30 May 2015

Received in revised form 11 June 2015

Accepted 11 June 2015

Available online 12 June 2015

Editor: J. Hisano

A B S T R A C T

Measuring the Higgs self-coupling is one of the crucial physics goals at the LHC Run-2 and other future colliders. In this work, we attempt to figure out the size of SUSY effects on the trilinear self-coupling of the 125 GeV Higgs boson in the MSSM and NMSSM after the LHC Run-1. Taking account of current experimental constraints, such as the Higgs data, flavor constraints, electroweak precision observables and dark matter detections, we obtain the observations: (1) In the MSSM, the ratio xMssm/x3M has been tightly constrained by the LHC data, which can be only slightly smaller than 1 and minimally reach 97%;

(2) In the NMSSM with X < 0.7, a sizable reduction of XNh2SSM/^Sh2 can occur and minimally reach 10% when the lightest CP-even Higgs boson mass m^ is close to the SM-like Higgs boson mh2 due to the large mixing angle between the singlet and doublet Higgs bosons; (3) In the NMSSM with X > 0.7, a large enhancement or reduction -1.1 < xN¡hMíSSM/x3¡^ < 2 can occur, which is accompanied by a sizable change of h-¡r+T- coupling. The future colliders, such as the HL-LHC and ILC, will have the capacity to test these large deviations in the NMSSM.

© 2015 The Authors. Published by Elsevier B.V. This is an open access article under the CC BY license

(http://creativecommons.org/licenses/by/4.0/). Funded by SCOAP3.

1. Introduction

With the discovery of the Higgs boson at the LHC [1,2], much effort has been devoted to study its properties. So far, the measurements of its couplings and quantum numbers are compatible with the standard model (SM) predictions at 1-2a level. However, to ultimately understand its nature, we need to fully reconstruct the Higgs potential at the LHC and future e+e- colliders [3,4]. The parameters in the Higgs potential determine the relations among the Higgs masses and self-couplings. Measuring these relations is therefore crucial for our understanding of the Higgs nature.

In the SM the tree-level Higgs potential is given by

V(0,SM) = -/x2(0t0) + k(0^0)2, 0 = — (0, v + h)T

which yields the following trilinear and quartic self-couplings

. (0,SM) Khhh

, (0,SM) Khhhh

* Corresponding author.

E-mail addresses: leiwu@physics.usyd.edu.au (L. Wu), jmyang@itp.ac.cn (J.M. Yang), yuan@pa.msu.edu (C.-P. Yuan), mczhang@itp.ac.cn (M. Zhang).

Here v = (V2Gf)-1/2 — 246 GeV is the vacuum expectation value of the Higgs field and mh — 125 GeV is the Higgs boson mass. Within the SM, the trilinear Higgs coupling receives the dominant correction from the top quark loop, SkSM — m^/(n2v2mj|) [5], which reduces its tree-level value by about 10%. Hence, the determination of the Higgs trilinear coupling khhh and quartic coupling khhhh can directly test the relation in Eq. (2) which is obtained from the minimization of the Higgs potential. At the LHC, the only way to measure the Higgs trilinear coupling is through the Higgs pair production, which is dominated by the gluon fusion mechanism and has a small cross section [6]. However, in many new physics models, such as the minimal supersymmetric model (MSSM) and the next-to-minimal supersymmetric model (NMSSM), the Higgs pair production rate can be significantly altered by new particles and Higgs couplings [7]. Among various decay channels of the Higgs pair, the 4b final state has the largest fraction [8], but the rare process hh ^ bbyy is expected to have the most promising sensitivity due to the low backgrounds at the LHC [9]. The recent applications of jet substructure and other techniques to Higgs pair production have been found to improve the sensitivity to the tri-linear Higgs couplings in t + t- and W+W- final states [10]. On the other hand, the measurement of the Higgs quartic coupling is more challenging due to a much smaller cross section of triple Higgs production at the LHC.

http://dx.doi.org/10.1016/j.physletb.2015.06.020

0370-2693/© 2015 The Authors. Published by Elsevier B.V. This is an open access article under the CC BY license (http://creativecommons.org/licenses/by/4.0/). Funded by SCOAP3.

The supersymmetric (SUSY) corrections to the Higgs self-coupling have two kinds of sources: one is the mixing between the Higgs bosons, and the other is radiative quantum effects. For the first kind, the authors in [11] studied the Higgs self-coupling in some simplified SUSY models, while in [12] the Higgs self-couplings in the MSSM and NMSSM (with a decoupled singlet boson) were investigated. Also, in [13] the authors studied the properties of the Higgs bosons in the NMSSM with X > 0.7 (called X-SUSY) and found a sizable enhancement in the Higgs self-coupling. For the second kind of SUSY corrections, the loop corrections to the Higgs self-couplings have been studied using the effective potential [14-22] or Feynman diagrammatic approach [23-25] in the MSSM and NMSSM. Recently, the leading two-loop SUSY-QCD corrections from the top/stop sector in the MSSM have been performed [26]. Since all these previous studies are limited to some simplified or special cases and the relevant experimental constraints are not fully considered, in this work we give a comprehensive study for the SM-like Higgs self-coupling in the MSSM and NMSSM with both X < 0.7 and X > 0.7 by considering all the relevant experimental constraints after the LHC Run-1.

The existing experimental data, both from low energy precision measurements and high energy direct searches, may have imposed important constraints on the Higgs self-coupling in SUSY models. For example, in the MSSM, the SM-like Higgs self-coupling is sensitive to the pseudo-scalar mass mA and tan p, which could have been tightly constrained by the LHC direct search of a light non-SM Higgs boson [27-29] as well as from precision B-physics [30]. Furthermore, the measured mass of the SM-like Higgs boson requires rather heavy stops and/or large Higgs-stop trilinear couplings, and the direct searches for the stop pair production have also pushed stop masses above hundreds of GeV in the natural SUSY [31]. Since the Higgs self-couplings are sensitive to stop masses and Higgs-stop trilinear couplings, all these constraints should be taken into account.

The structure of this paper is organized as follows. In Section 2, we will briefly describe the Higgs sectors of MSSM and NMSSM. In Section 3, we perform a scan over the parameter space of each model and present the numerical results for the trilinear self-coupling of the SM-like Higgs. Finally, we draw our conclusions in Section 4.

2. Higgs trilinear self-couplings in MSSM and NMSSM

21. Higgs trilinear self-couplings in the MSSM

In the MSSM there are two doublets of complex scalar fields with opposite hypercharges:

The scalar Higgs potential consists of the D-terms and F-terms of the superpotential as well as the soft SUSY-breaking mass terms. Among them, the D-terms determine the quartic Higgs interactions. The full tree-level Higgs potential is given by

V (0,MSSM) = m2,Hu |2 + m2|Hd |2 - B߀aß(Ha Hß + h.c.)

g2 + g2

(IHu |2 -|Hd|2)2 + ^ |HUHd|2

where eap is the antisymmetric tensor and m^ 2 = m2H + j2 with mHu d and j denoting the soft SUSY-breaking masses and the hig-gsino mass, respectively. The parameters m1 2 can be eliminated by the minimization condition of the Higgs potential, while the

parameter Bj is traded for the pseudoscalar mass MA. The quartic Higgs couplings are fixed in terms of the SU(2) x U (1) gauge couplings g and g' in the MSSM.

After the electroweak symmetry breaking, the neutral components of the two Higgs fields Hu0 d develop vacuum expectation values (vevs) vu,d and can be decomposed into scalar and pseu-doscalar components as

Re H0 = (vd + Hca - hsa)/V2, Im H0 = (G0Cß - Asß)/V2,

Re HU = (vu + Hsa + hca)/V2, Im Hu = (GUsß + Acß)/^2

where h, H and A are the neutral physical Higgs bosons and G0 is the would-be Goldstone boson. The vevs are defined as Vu — vsp and Vd = vcp with v & 246 GeV (here and in the following we use the notation cx = cos x, sx = sin x). Taking the third derivatives of

V (0,MSSM)

with respect to the

physical Higgs fields yields the trilinear Higgs couplings. In the physical mass eigenstates, the neutral CP-even Higgs trilinear couplings at leading order are given by

(0,MSSM) _ 3M1

c2a sa+ß,

, (0,MSSM) M1 rn ,

XHhh = [2s2asa+ß - c2a ca+ß i, , (0,MSSM) _ 3M1

(0,MSSM)

c2a ca+ß,

( , ) 1 XHHh =--- ca+ß + c2a sa+ß

In the MSSM, either the lighter scalar h or the heavier scalar H can be the SM-like Higgs boson. The latter interpretation occurs for low values of MA (between 100 and 120 GeV) with moderate values of tan /) (about 10). In this case, H has approximately SM-like properties, while the other four Higgs bosons of the MSSM would be rather light and have a mass of order 100 GeV or even below. A dedicated scan for this region of parameter space has been performed in [32] and it was found that this scenario can be excluded by recasting the LHC search for H/A ^ t+t- [27]. In addition, the latest ATLAS limits from H± searches have also excluded such a possibility [29]. Thus, in this work, we will only study the case that h is the SM-like Higgs boson in the MSSM. According to Appelquist-Carazzone decoupling theorem, the MSSM must go back to the SM in the decoupling limit. In the tree-level Higgs sector, we can make this limit by setting mA ^ ro, which gives a ^ /) — y. Applying this relation to the first identity in Eq. (7) yields

(0,MSSM) hhh

3M 1c2

h,(0,MSSM)

where mh,(0,MSSM) — MZc2p is the lighter CP-even Higgs mass at tree-level. This demonstrates that the lighter Higgs boson h in the MSSM almost behaves like the SM Higgs boson in the decoupling limit (even when the loop corrections are included) [23,24].

2.2. Higgs trilinear self-couplings in the NMSSM

After the discovery of a 125 GeV Higgs boson, the NMSSM [33] seems to be more favored than the MSSM because it can naturally give such a Higgs boson without very heavy top-squarks [34]. More importantly, this model can solve the ¡-problem: after the singlet field develops a vev (S) = vs/V2, an effective ¡-term

(—eff = kvs/42) is dynamically generated. Due to the contribution of the singlet scalar field S, the full tree-level Higgs potential can be written as

O2a + O2a + O3a = 1-

V (0,NMSSM) = (|k S |2 + m2Hu )HU Hu

2 TY1 Mft

+ (|kS|2 + mHd )Hd Hd + m2S | S |2

+ 8 (g2 + g2)(Hu Hu - Hd Hd )2 + 2 g21H lHd |2

+ |eadkHau + kS2|2

+ [<sadkAkHaHpd S + 1 kAk S3 + h.c.], (10)

where k and k are dimensionless parameters, and Ak and Ak are the corresponding trilinear soft breaking parameters. To clearly show the properties of the Higgs sector, we can expand the neutral scalar fields around the vevs as [33]

Re H0 = (vd - H sin d + h cos d)/^2, Im H0 = (P sin d + G0 cos d)/42, Re H0 = (vu + H cos d + h sin d)/^2, Im H0 = (P cos d - G0 sin d)/ V2, Re S = (vs + s)/42,

Im S = Ps/42. (11)

Substituting Eq. (11) into Eq. (10), we obtain the mass matrix squared M2S for the neutral CP-even Higgs bosons and the trilin-ear Higgs self-interactions as

g-2' H¡H .'2

/(0,NMSSM) CP-even

= - (H, h, s) M2SI h + khahdhy hahdhy, (12)

with ha,d,Y = H, h, s. The tree-level M|.. are given by [35]

MS n = M2A + (MZ - 2k2 v2) sin2 2d,

MS12 = - (MZ - 1 k2 v2) sin4d,

M S13 = -42kv —x cot2d,

MS 22 = M2Z cos2 2d + 2k2 v2 sin2 2d, MS 23 = V2kv—(1 - x), 2

'S 23 2

(16) (17)

. k2 2 k k2v2 Kk 2 , ,

M2s 33 = 4k2 fi + k AkI + — x - — v sin 2d, (18)

(V2Ak + kv^ , x = 2-(Ak + 2K-f)-

sin 2d V' k ' s^ 2— k ' ^ ' ' ()

Here, it should be mentioned that the mass parameter MA in the NMSSM becomes the mass of the heavy pseudoscalar Higgs boson only in the MSSM limit (k, k ^ 0 with the ratio K/k fixed). In the NMSSM, MA can be traded by the soft parameter Ak.

The CP-even Higgs mass eigenstates hi (i = 1, 2, 3) can be obtained by diagonalizing MS with a rotation matrix O

hi = Oiaha, (ha = H, h, s), diag(m2], m22, m23) = OM2sOT

with Oia being the elements of the rotation matrix satisfying the sum rules

The mass eigenstates hi are aligned by the masses mh, < mh2 < mh3 . The singlet or non-SM doublet components in a physical Higgs boson hi is determined by the rotation matrix elements Oi(H,s). With Eq. (20), the corresponding tree-level trilinear Higgs couplings in the mass eigenstates hi are given by

,(0,NMSSM) n n n , khihjhk = OiaOjdOkykhahfihy -

In the NMSSM, we take h1 or h2 as the SM-like Higgs boson when |O(12)h|2 > 0.5. In general, due to the introduction of the singlet s and its couplings to the MSSM Higgs sector, the mass of the SM-like Higgs boson M S can be lifted by the extra large k-term at tree level, as shown in Eq. (16). The value of k at the weak scale is upper bounded by 0.7 in order for the NMSSM to remain perturbative up to the GUT scale [33,35]. Whereas, the case of k > 0.7 (dubbed as k-SUSY model) is still of interest because it can suppress the sensitivity of the Higgs mass with respect to changes of the soft SUSY-breaking masses and keep the fine tuning at a moderate level even for stop masses up to 1 TeV. So, in our study, we consider both k < 0.7 and k > 0.7 cases:

• For k < 0.7, in addition to the tree-level k contribution, the mixture of the singlet s with the MSSM Higgs h and H, as shown in Eq. (13), in particular with h, could further modify the SM-like Higgs mass. If H is decoupled, when MS > MS33, the mass eigenvalues for the SM-like Higgs boson mh2 is pushed up by the positive mixing effect after the diagonaliza-tion of the h - s mass matrix. However, when M? < M? , the

' s— S33'

mass eigenvalues for the SM-like Higgs boson mh1 is pulled down by the negative mixing effect. Without the negative mixing effect, the maximal tree-level SM-like Higgs mass mh1 can only reach to about 110 GeV [36,37], which needs a sizable loop correction from the stop sector to obtain a 125 GeV Higgs boson like in the MSSM. In this sense, h2 being the observed SM-like Higgs boson may be more natural than h1 in the NMSSM. So, we choose the next-to-lightest CP-even Higgs boson h2 as the SM-like Higgs boson in the following discussions for the NMSSM with k < 0.7. Note that the lightest Higgs boson h1 in this case is predominantly singlet-like and its mass can be as light as about 20 GeV in our scanned samples. Consequently, the SM-like Higgs boson h2 can decay into a pair of light scalars h1 and hence the yy and ZZ* signal rates are suppressed. In order to be consistent with the LHC Higgs data, the branching ratio of h2 ^ h1h1 was found to be less than about 30% [38] and may be tested through h1h1 ^ bb—+ -production channel at the 14 TeV LHC [39]. However, due to our interests in the large mixing region, we only display the results with mhj > mh2/2 in the following analysis. We will also decouple the heaviest CP-even Higgs boson h3 by requiring mh3 > 1 TeV and focus on the singlet-doublet system. On the other hand, as mentioned above, if h1 is the SM-like Higgs boson, the value of k tends to be large in order to maximize the tree-level Higgs mass (so in our study for k-SUSY with k > 0.7, we will choose h1 as the SM-like Higgs boson). This feature may lead to a sizable change in Higgs self-coupling when doublet-singlet mixing effect is large. We checked this possibility and found that the ratio k3NhMSSM/kS3Mh can vary from 0.29 to 1.17 for our samples with k < 0.7.

• For k > 0.7, we choose the lightest CP even Higgs boson h1 as the SM-like Higgs boson. The reason is that for k > 0.7 the tree-level Higgs mass will be significantly lifted. If h2 is assumed as the SM-like Higgs boson, the large k-term in MS and the positive doublet-singlet mixing effect can readily

make the SM-like Higgs mass mh2 exceed 125 GeV. Thus, such a choice is strongly disfavored by the LHC observed Higgs mass [37] and will not be further studied in our work. If hi is the SM-like Higgs boson, as pointed before, the cancellation between the tree-level X-term and the negative doublet-singlet mixing effect can easily yield a 125 GeV SM-like Higgs boson. However, X cannot be too large, because the large trilinear and quartic couplings of singlet scalar field s will largely contribute to the scattering amplitude ss ^ ss. In the high energy limit, the unitarity condition requires |X| < 3 and |k| < 3. Furthermore, if combined with the dark matter relic abundance constraint, the above-mentioned unitarity bound can set a generic upper bound 20 TeV for the heavy Higgs masses [40]. The requirement of perturbativity up to the cut-off scale A, i.e., X(A) < 2n and k(A) < 2n, will set upper bounds on X and k at weak scale. In this study, we assume the new unknown strong dynamics, for restoring the unitary of scattering processes, appears at some scale A above 10 TeV, and require X2 + k2 < 4.2 [35,41].

Before closing this section, we note that since both Higgs boson masses and Higgs self-interactions arise from the Higgs potential, one has to adopt the same method to calculate them up to the same order for comparing the self-couplings in SUSY and SM. Although the most accurate evaluation of Higgs mass is up to three-loop level in the MSSM [42], there is no corresponding result for the Higgs self-couplings. Hence, in our study, we derive the Higgs mass and self-couplings by following the effective potential approaches in the MSSM [14] and NMSSM [21], where the explicit dominant one- and two-loop corrections to the effective potential are presented. Then we coded those expressions in our numerical calculation. On the other hand, since the tree-level mixing effects in the Higgs sector are usually dominant over the loop corrections in the NMSSM, we will focus on the doublet-singlet mixing effects for the NMSSM results.

3. Numerical calculations and results

31. Scan over the parameter space

In our numerical calculations, we take the input parameters of the SM as [43]

mt = 173.5 GeV, mW = 80.385 GeV, mZ = 91.1876 GeV,

mMS(mMS) = 4.18 GeV, as(MZ) = 0.1184,

a(mZ)—1 = 128.962 (23)

We use NMSSMTools-4.4.1 [44] to perform a random scan over the parameter space. Note that for any given value of ¡eff, the phenomenology of the NMSSM is identical to the MSSM in the limit X, k ^ 0 with the ratio k/X fixed (Ak should be negative and satisfy | Ak | < 4kj/X to guarantee the squared mass of the singlet scalar to be positive) [33]. In our scan for the MSSM, we take X = k = 10—7 and Ak = —10 GeV. The validity of such a method has been justified by the authors of the NMSSMTools [44] and our previous calculations [34]. We also numerically checked our MSSM results of mh by using the codes FeynHiggs [45], SOFTSUSY [46] and SuSpect [47], and found the results to agree with that given by the NMSSMTools within about 1% level when mh ~ 125 GeV. So it is feasible to use the package NMSSMTools in the MSSM limit to study the phenomenology of the MSSM. For simplicity, we decouple the sleptons, gauginos and the first two generations of squarks by fixing the corresponding soft mass parameters at 2 TeV. We also set Mq3 = MD3 = MU3 and At = Ab for the third generation

of squarks. The lower limit of tan $ in the MSSM is taken as 5, which is inspired by the recent LHC Higgs results [32]. The parameter ranges in our scan are chosen as the following:

(a) For the MSSM,

5 < tan $ < 60, 0.2 TeV < MA < 1 TeV, \f\ < 1 TeV,

0.1 TeV < MQ3 < 2.5 TeV, \At\< 3MQ3. (24)

(b) For the NMSSM with X < 0.7,

0 < X < 0.7, \k \< 0.7, 0.2 TeV < AX < 1 TeV,

\ AK \ <1 TeV, 1 < tan $ < 20, 0.1 TeV < fi < 1 TeV,

0.1 TeV < MQ3 < 1 TeV, \ At\ < 3MQ3. (25)

(c) For the NMSSM with X > 0.7,

0.7 < X < 2, 0 <k < 2, 0.2 TeV < AX < 1 TeV,

\ AK \ <1 TeV, 1 < tan $ < 20, 0.1 TeV < fi < 1 TeV,

0.1 TeV < MQ3 < 1 TeV, \ At\ < 3MQ3. (26)

In our scan, we consider the following constraints:

(1) We require the SM-like Higgs mass in the range of 123127 GeV and consider the exclusion limits (at the 95% confidence level) from LEP, Tevatron and LHC in Higgs searches with HiggsBounds-4.2.0 [48]. We also perform the Higgs data fit by calculating x2 of the Higgs couplings with the public package HiggsSignals-1.3.0 [49] and require our samples to be consistent with Higgs data at 2a level. We choose the SLHA input choice of HiggsBounds/HiggsSignals, where the effective Higgs couplings are only used to calculate the Higgs production cross section ratios. The Higgs decay branching ratios are taken directly from the corresponding decay blocks in the SLHA file generated by the NMSSMTools.

(2) We require one-loop SUSY predictions for B-physics observables to satisfy the 2a bounds as encoded in NMSSMTools,

which include B ^ Xsy, Bs

Bd ^ Xsf+f and

b+ ^ t +v. Theoretical uncertainties in B-physics observables are taken into account as implemented in NMSSMTools.

(3) We require the one-loop SUSY predictions for the precision electroweak observables such as pi, sin2 8leff, mW and Rb [50] to be within the 2a ranges of the experimental values.

(4) We require the thermal relic density of the lightest neutralino (as the dark matter candidate) is below the 2a upper bound of the Planck value [51] and the spin-independent neutralino-proton scattering cross section satisfy the direct detection bound from LUX at 90% confidence level [52].

(5) We also consider the theoretical constraints from the stability of the Higgs potential as encoded in the NMSSMTools.

3.2. Results for the MSSM

Precision measurements of the Higgs boson properties (its mass and couplings to other particles) at the LHC provide relevant constraints on possible weak-scale extensions of the SM. In the usual context of the MSSM, these constraints suggest that all the additional non-SM-like Higgs bosons should be heavy. In Fig. 1, we show that in the decoupling limit of the MSSM, the region with mA < 330 GeV has been excluded by various constraints. Similar result has been recently pointed out in [53]. The lower part of Fig. 1 shows that the value of tan /) cannot be too small due to the requirement of 125-127 GeV Higgs mass in our scan. For

150 200 250 300 350

MA (GeV)

Fig. 1. Excluded region in the tan p versus MA plane of the MSSM.

a small tanp, heavy stops (>10 TeV) or a large mixing parameter At is needed to produce a large positive correction to the Higgs mass, which, however, will easily lead to vacuum instability and large uncertainty in the numerical calculation. So, we focus on m~ti < 2.5 TeV region in our calculations. The additional constraints on the MSSM parameters imposed by the Higgs data are obtained by using the HiggsBounds-4.2.0 package. The key algorithm of HiggsBounds can be described in two steps. Firstly, the HiggsBounds uses the expected experimental limits from LEP, Teva-tron and LHC to determine which decay channel has the highest statistical sensitivity. Secondly, for this particular channel, the theory prediction is compared to the observed experimental limits to conclude whether this sample is allowed or excluded at 95% CL. With the HiggsBounds, we find that most of samples (black bullets) with 180 < MA < 330 GeV and 5 < tan P < 10 have been excluded. Particularly, the latest CMS result of searching for H/A — t +t — has excluded most parameter space with a low MA and low to moderate values of tan p, as shown in the upper left corner of Fig. 1. We have checked that the current low energy constraints from Bs — ¡i+ and Bs — Xs y are weaker than H/A — t +t — for our interested region (low to moderate values of tan p). We note that the supersymmetric loop corrections generally lead to a contribution of the order of a few percent of the SM value. Hence, the suppressions in Higgs signal strengths ¡iyy and \xVV* are mostly governed by the increase of the width of the lightest CP-even Higgs decay into bottom quarks and tau leptons at low values of mA.

Fig. 1 suggests that all the additional non-SM-like Higgs bosons should be heavy, with masses larger than about 330 GeV. This is the commonly discussed decoupling limit of the MSSM. However, as discussed in [54], it is also possible to have the MSSM parameter conditions for "alignment independent of decoupling", where the lightest CP-even Higgs boson has SM-like tree-level couplings to fermions and gauge bosons, independently of the non-standard Higgs boson masses. In the alignment region, sin(a — P) ~ 1 and the bounds on the heavy Higgs bosons that arise from the measurements of h — VV may be relaxed. Such alignment conditions are associated with very SM-like htt coupling and tend to be restricted to values of tan p of order 10 or larger within the MSSM [54-56]. As will be shown below, for such a large value of tan p, the supersymmetric contributions to the SM-like Higgs self-coupling are found to be small (at a percent level). Hence, even in the alignment condition, we cannot expect a large deviation of the Higgs self-coupling with the SM value.

In Fig. 2 we project the samples surviving all the experimental constraints on the planes of mA and m-t1 versus tan p. The ratio ^MhiSM/^3M is always smaller than 1 because of the negative MSSM corrections to Higgs self-coupling [23]. From the left panel it can be seen that in most part of the allowed parameter space (the blue triangles), the values of ^MhSSM/^S3M (we use 3h to denote hhh) are larger than 0.99. When both tanp and mA become small, ^MhSM/^3M gets smaller, which can minimally reach about 0.97 for our samples. The reasons for XMShM being so close to ^3M are the following: (1) The dominant MSSM contributions to xMSSM/x3^ are from the stop loops, while the Higgs coupling with the stops is proportional to 1/ sin p. So it leads to an overall enhancement factor 1 / sin3 p in the corrections when tan p is small. However, such a region is obviously not favored by the measured Higgs mass, which needs a large tan p to enhance the Higgs mass; (2) A light mA causes a large mixing between two CP-even Higgs bosons and can sizably change the Higgs couplings with the SM fermions. But as mentioned before, mA should be heavier than about 330 GeV to satisfy the experimental constraints in our scan. For the right panel it should be mentioned that since the small values of XMfhhMA3M occur in the small tan p region, heavy stops are usually needed to enhance the Higgs mass through loop corrections.

In Fig. 3, we show the MSSM Higgs couplings in comparison with the SM predictions. The ILC (1 TeV, 1 ab—1) sensitivities to the alteration of the couplings [57] are also plotted, where the regions between the bars give too small alterations to be detectable at ILC. The HL-LHC (14 TeV, 3 ab—1) sensitivities are much worse than ILC and are not shown here. From Fig. 3, we have the following observations: (1) In the MSSM, the Higgs gauge couplings and top-Higgs couplings are respectively changed by the factors sin(p — a) and cos a/ sin p, but the ratios cMVSM/csMV and C^/C™ for our survived samples are very close to unity due to mA ^ mZ. So, even if these couplings can be measured at percent level at ILC, it cannot constrain the MSSM parameter space with a small ^MhSM/^3M; (2) The ratio cMghghM/C^g is always smaller than one for our samples because a large mixing between the stops or heavy stops needed by the Higgs mass interferes destructively with the top loop and cMSgSM is suppressed, while CMSSM/ChMy can be greater than one due to the constructive contribution with the W loop. Although both couplings only slightly deviate from the SM predictions, the high precision measurements on Cgg,yy at the ILC will be able to exclude some part of the parameter space with xMhhMA3if > 0.977.

3.3. Results for the NMhhM (X < 0.7)

In Fig. 4, we project the NMSSM (X < 0.7) samples allowed by the constraints (1)-(5) on the planes of X versus k and k versus the singlet component |O2s| in the SM-like Higgs boson h2. Here we take 2mh1 > mh2 so that h2 will not decay into a pair of h1. We can see that when X and k approach to zero, tan p has to be large in order to enhance the Higgs mass. While in small tan p < 10 region, the values of X for most samples are larger (in magnitude) than k. Since the singlet component lO2s| in the SM-like Higgs boson h2 can potentially affect the Higgs self-coupling in Eq. (22), we also show the dependence of |O2s |. Since the singlet component |O2s| in the SM-like Higgs boson h2 can potentially affect the Higgs self-coupling in Eq. (22), we also show the dependence of |O2s| on X and k for the NMSSM (with X < 0.7) samples which survive all the experimental constraints. It can be seen that |O2s | deceases if both X and k go to zero. However, if X ^ ! | ~ 0, which usually happens for small tan p < 10, |O2s| can be sizeable and lead to a large deviation from the SM prediction in triple Higgs boson cou-

0.4 0.5 0.6 0.7 0.8 0.9 1 0.6

M, (TeV)

0.9 1.2 1.5 1.8 2.1 2.4

M7i(TeV)

Fig. 2. Scatter plots of the samples surviving all the experimental constraints, projected on the planes of tand versus mA and m^. (For interpretation of the references to color in this figure legend, the reader is referred to the web version of this article.)

jMSSM/JSI

Ah. '■rt'M

K | 1.00

ILC(1TeV, lab-1)'

fMSSM,£SM hW hW

0.96 0.98 1.00 1.02 1.04

fMSSM/f^SM "39 hgg

Fig. 3. Same as Fig. 2, but showing the Higgs couplings. The ILC (1 TeV, 1 ab ') sensitivities to the alteration of the couplings [57] are also plotted (the regions between the bars give too small alterations to be detectable at ILC).

1.0 -1-1-1-1-1-1-1-1-1-1-1-1-1-1-1-1 4U U.U-|-1-1-1-1-1-1-1-1—r T—i^T"'-1-1-I

0.0 0.1 0.2 0.3 0.4 0.5 0.6 0.7 0.8 -0.8 -0.6 -0.4 -0.2 0.0 0.2 0.4 0.6 0.8

Fig.4. The NMSSM (k < 0.7) samples surviving all the experimental constraints, projected on the planes of k versus k and the singlet component |02s| in the SM-like Higgs boson h2.

-0.6 -0.4 -0.2 0.0 0.2 0.4 0.6

Singlet component IOJ in h2

Fig. 5. Same as Fig. 4, but showing the dependence of xNM2 /x3M versus X and the singlet component |02s| in h2, where m^2 < 2m/11. The ILC (1 TeV, 1 ab 1) and HL-LHC (14 TeV, 3 ab-1) sensitivities are also plotted (the region below each horizontal line is detectable).

pling. For example, for X = 0.017 and k = —0.0038, O2s ~ 0.215 and XNhf2hhMXM ~ 0.7. The reason is that in the singlet-doublet system, after decoupling h3 by requiring Mh3 > 1 TeV, |O2s | is proportional to sin 6, where the mixing angle 6 that determines the mixture of the singlet and the SM-like Higgs states can be approximately expressed as tan26 ~ 2M23/(M22 — M|3) [35,37]. Here, M2. are the CP-even Higgs mass matrix elements listed in Eqs. (13)-(18). In case that X is not too small, a large 6 can happen when M|2 — m33 ~ M23. This leads to a large singlet component in the SM-like Higgs state and hence a sizeable modification of the Higgs trilinear couplings.

In Fig. 5, we display the dependence of XNMhhM/XhM versus X and tanp for the NMSSM (X < 0.7). As mentioned above, due to the Higgs mass constraint, most of the allowed model samples tend to have large values of X. Furthermore, the ratio XNM2hhM/XhM is not sensitive to the value of tan p. We also show the dependence of XNM2hhM/X3M versus the singlet component |O2s| in the SM-like Higgs boson h2 and the lightest CP-even Higgs mass mh1 for the NMSSM (X < 0.7). Besides, we plot the expected ILC (1 TeV, 1 ab—1) and HL-LHC (14 TeV, 3 ab—1) sensitivities to Higgs self-coupling from the direct measurements [57]. We can see that XNNM2hhM/X3M becomes small with the increase of the singlet component |O2s | and can minimally reach 0.1 in the allowed parameter space. Meanwhile, such a large mixing can make the mass of the lightest singlet-dominant CP-even Higgs boson h1 close to the 125 GeV SM-like Higgs boson h2.

In Table 1, we present the properties of two CP-even Higgs bosons h1 and h2 for such a benchmark point at 14 TeV LHC. We can see that the cross sections of the single h1 production are close to those of SM-like h2 because of the large doublet and singlet mixing components in both h1 and h2. However, the branching ratio h1 — VV (V = Z, Wy, g) is greatly suppressed by the increase of the partial width of h1 — bb. Thus, the observed production rate of gg — h1 — VV is much smaller than that of SM-like h2. We also checked and found that although the cross section of gg — h1 — t + t — can reach 2.06 pb, it is still smaller than the upper bound given by the current LHC searches for H / A — t + t— [28]. Besides, it should be mentioned that the sizable modification of the self-coupling of the SM-like Higgs boson h2 always accompanies with the great changes in other Higgs couplings, which can be seen in Fig. 6. So, given the limited sensitivity of measuring the

Higgs boson self-couplings, we anticipate that the precision measurement of Higgs couplings to gauge bosons and fermions could test this scenario at the LHC and future colliders prior to the direct detection of triple or quartic Higgs couplings.

In Fig. 6, we show the Higgs couplings in the NMSSM (X < 0.7) surviving all the experimental constraints. For comparison, we also show the discovery potential of the expected ILC (1 TeV, 1 ab—1) and HL-LHC (14 TeV, 3 ab—1) [57]. From this figure, we obtain the following observations: (1) Due to the singlet admixture in the SM-like Higgs boson, both Higgs gauge couplings and top-Higgs coupling can be maximally reduced by about 30% in the allowed region, which is much larger than in the MSSM. So, the expected measurements of the Higgs gauge couplings at the HL-LHC and ILC can exclude the parameter space with XNM2hhM/XS3M < 0.82 and XN3M2hhM/X3M < 0.93, respectively; (2) With the increase of the singlet component in the Higgs couplings, both ChNgMghhM/ChhMgg and cNMSsm/cSMy are significantly reduced. On the other hand, due to the additional tree-level contribution (~Xv sin2p) and the positive mixing effect, we find that a stop with mass less than 200 GeV is still allowed by the SM-like Higgs mass constraint in the NMSSM (similar results have been obtained in previous NMSSM works [58]). Consequently, the ratio ChNgMghhM/ChhMgg becomes larger than one, due to the constructive contribution from the light stop in loop. We also note that even when X3NhMhhM approaches to

X3M, CN!MMM/cSMy can still be enhanced by about 8%.

NMhhM / j hM

3.4. Results for the NMhhM (X > 0.7)

In Fig. 7, we display the dependence of X tanp and mh2 for the NMSSM (X > 0.7). Similar to Fig. 4, the larger X is, the smaller tan p becomes to satisfy the requirement of the Higgs mass. The ratio XNMhhMA3M can vary from —1.1 to 1.9 in our scan. For example, the ratio XNMthhM/X3M is equal to 1.89 when X = 1.51 and k = 0.67, and is —1.04 for X = 1.57 and k = 1.16. Since we require mh3 > 1 TeV, for our samples with mh3 » mh12, X33MlhhM/X3M is approximately proportional to X2 and becomes large with the increase of X. In our scan ranges, such a feature could either enhance or suppress the Higgs self-coupling with respect to the SM prediction, and yield potentially large effects in Higgs

Table 1

A benchmark point for the NMSSM with X < 0.7 (h2 is the SM-like Higgs boson). The cross sections (pb) are calculated for LHC-14 TeV.

X K tan p I (GeV) Ax (GeV) Ak (GeV) -.NMSSM r,i X3h2 'X:

0.16 0.31 17.9 105.3 1461.9 -716.2 0.798

mh1 (GeV) °ggh\ aVVh, aWh1 &Zh\ °tih, abbh,

119.56 25.41 2.14 0.85 0.49 0.33 0.54

Brh^Y y Brhi^gg Brh,^ZZ * Brh1 ^WW * Brh1 ^cc Brh^bb Brh,^r +T-

0.135% 3.60% 0.717% 7.88% 2.12% 77.3% 8.10%

mh2 (GeV) °ggh2 OVVh2 OWh2 ®Zh2 atih2 abbh2

127.30 24.81 2.05 0.71 0.41 0.29 0.14

Brh2^Y Y Brh2^gg Brh2^ZZ * Brh2 ^WW * Brh2 ^cc Brh2^bb Brh2^T +r-

0.381% 8.11% 3.92% 34.0% 4.14% 44.6% 4.55%

HL-LHC(14TeV, Sab"1)

ILC(1TeV, lab"1)

X<0.7,

L. SM-like I

*NMSSM/«SM

3h, 3h

. HL-LHC(14TeV, 3ab"')

ILC(1TeV, lab-1

0.8 0.9 1.0 1.1 0.6 0.7 0.8 0.9 1.0 1.1 1.2

fNMSSMf^NMSSU

hgg hgg

Fig. 6. Same as Fig. 3 but for the NMSSM (X < 0.7).

. ,HL-LHC(14Tey,3ab^pjrect Detection) .

. _ !LCOTeVJab-\pireet^etoction)_ • *

¿>0.7,

11 13 15

mh2 (GeV)

Fig. 7. The NMSSM (X > 0.7) samples surviving all the experimental constraints, showing the dependence of X™ A3™ versus tanp and mh2. The ILC (1 TeV, 1 ab 1) and HL-LHC (14 TeV, 3 ab-1) sensitivities are also plotted.

m to (GeV)

mhi (GeV)

Fig. 8. The NMSSM (X > 0.7) samples surviving all the experimental constraints, showing the dependence of the Higgs couplings versus mh2.

Table 2

A benchmark point for the NMSSM with X > 0.7 (hi is the SM-like Higgs boson). The cross sections (pb) are calculated for LHC-14 TeV.

X K tan ß ß (GeV) ¿x (GeV) AK (GeV) -.NMSSM r.i x3h2 'x:

1.54 0.75 3.06 474.00 1035.41 -644.30 -0.203

mhi (GeV) agghi °VVh1 ®Wh1 OZh1 atih1 abbh1

126.9 42.86 3.42 1.17 0.70 0.52 0.29

Brhi ^y y Brhi^gg Brh1 ^ZZ * Brh1^WW * Brhi^cc frhi^bb Brhi^T +T-

0.427% 9.87% 4.18% 36.5% 4.98% 39.7% 4.03%

mh2 (GeV) aggh2 °VVh2 ®Wh2 OZh2 °tth2 abbh2

282.0 6.33 0.90 0.06 0.03 0.03 0.04

Brh2 ^y y Brh2^gg Brh2 ^ZZ * Brh2^WW * Brh2^bb Brh2^r+r - Brh2^hihi

0.000663% 0.0173% 14.1% 32.1% 0.0996% 0.012% 53.6%

pair production cross sections [13,59]. However, in general, the two masses m^2 and m^3 are virtually independent and the mixing patterns are complicated. It is worth mentioning that the value of XN3MSSM/X3M ^ 1 strongly relies on the mass of the next-to-lightest CP-even Higgs boson h2. To be specific, when k becomes small (large), mh2 is inclined to be light (heavy). If mh2 is lighter (heavier) than about 400 GeV, X3NMSSM1X3™ is smaller (larger) than unity for most samples. The properties of h2 will be discussed in the following. We should mention that the large X and k that produce the large deviation of xNMfSM/x3M jeopardize the perturbativity up to GUT scale. Thus, the new unknown strong dynamics will appear at some cut-off scale A. On the other hand, the constructions of high scale theory by adding vector-like matter can allow for a larger X value and relax the cutoff scale to high values [60], which is however beyond the scope of our study.

In Fig. 8, we plot the couplings of h2 with gauge bosons and t leptons, normalized to the SM values. We can see that the gauge coupling h2 VV is always suppressed due to the presence of singlet (s) and non-SM doublet (H) components in h2. If h2 is singlet-like, the h2T+t- coupling is suppressed as well, while if h2 is non-SM doublet-like, h2T+t- coupling can be enhanced by tanp. The detailed mixing patterns of s and H in h2 and its couplings have been thoroughly investigated in [59]. We checked that the cross section gg ^ h2 ^ t + t- for our samples is at least one order lower than the current direct search bound on the non-SM Higgs bosons [27, 28]. The main reason is that for a heavy Higgs boson h2, the new

decay channels, such as h2 ^ h1h1 [61], can be opened and the branching ratio of h2 ^ t+ t + will be highly suppressed.

In Table 2, we present the properties of two CP-even Higgs bosons h1 and h2 for a benchmark point at 8 TeV LHC. We can see that all the SM branching ratios of h2 are reduced due to the opened decay mode h2 ^ h1h1, which can reach 53.6% for mh2 = 282.0 GeV. Such a Higgs-to-Higgs decay will lead to a resonant SM-like di-Higgs bosons production pp ^ h2 ^ h1h1 at the LHC. A resonance feature in the h1 h1 invariant mass can be served as a smoking gun to search for the heavy Higgs boson h2. With one SM-like Higgs boson h1 decaying to two photons and the other decaying to b-quarks, the resonant signal may be observable above the di-Higgs continuum background for mh2 < 1 TeV at the HL-LHC [62].

Next, we present in Fig. 9 the couplings of the SM-like h1 to weak gauge bosons and tau pair for the NMSSM (X > 0.7). To show their correlation with the Higgs self-coupling, we use the red color to highlight the points that satisfy |XNMSSM/X3™ - 1| > 0.3. It can be seen that the large Higgs self-couplings corrections correspond to the sizable shifts in Higgs couplings with gauge bosons and tau pair. Since the tree-level mass of the SM-like Higgs boson h1 could easily exceed 125 GeV, h1 is likely to have non-negligible singlet and/or non-SM doublet components, which makes its couplings deviate from the SM predictions. From this figure, it can be seen that cNMvVM/ChMv is always less than unity since any singlet and/or non-SM doublet components in h1 will make the Higgs couplings to weak gauge bosons smaller than the SM pre-

1.2 1.1 1.0

« I 0.9

« 0.8

V 07 0.60.50.4-

(0.7, 1.3) ánmssmiáSH 3 (1 3i 1 _ о 7)

:(14TeV, 3ab

X > 0.7, /if

^NMSSM/^SM h.W hw

Fig.9. Same as Fig. 8, but showing the couplings of hi. The HL-LHC (14 TeV, 3 ab 1) and ILC (1 TeV, 1 ab-1) sensitivities [57] are also plotted.

dictions. However, as mentioned above, if the next-to-dominant component in h1 is the non-SM doublet, the Higgs coupling with the down-type fermions may be enhanced and larger than the SM predictions, such as the h1T + t- coupling. Therefore, the future measurements of Ch1T+t- and Ch1 vv couplings can give strong constraints on the parameters space of the NMSSM with X > 0.7 and set limits on the Higgs self-coupling C3NhMSSM.

From the above discussions, we can see that the large deviation of the Higgs self-coupling X3h1 for the NMSSM (X > 0.7) is always accompanied by other collider signatures, such as a shift in the Higgs couplings and the production on resonance of the non-SM doublet h2. At the LHC, the resonant production of h2 may be observed through the channels gg ^ h2 ^ t + th1h1. However, the sensitivities of these channels strongly depend on the mass of h2 and on its singlet and non-SM doublet components. If h2 is dominantly singlet, both direct searches will not be powerful in probing our scenario at the LHC since all the h2 couplings to SM particles are greatly reduced. Thus, the precision measurement of the observed 125 GeV Higgs boson couplings will play a unique role in probing this scenario at future colliders. If h2 is domi-nantly doublet (non-SM), and if mh1 < mh2 < 2mh1 , the process gg ^ h2 ^ t+t- is still greatly suppressed due to the reduction of the coupling h2tt despite the fact that the coupling h2 t +t- can be maximally enhanced by a factor of 2. On the other hand for 2mh1 < mh2, the decay h2 ^ h1h1 is open and contributes to the cross section of pp ^ h1h1. Therefore, besides the Higgs coupling measurements, a resonance feature in the h1 h1 invariant mass or an excess in the inclusive h1 h1 production can be used to probe this model at the future LHC.

4. Conclusion

We examined the currently allowed values of trilinear self-couplings of the SM-like 125 GeV Higgs boson (h) in the MSSM and NMSSM after the LHC Run-1. Considering all the relevant experimental constraints, such as the Higgs data, the flavor constraints, the electroweak precision observables as well as the dark matter detections, we performed a scan over the parameter space of each model and obtained the following observations:

• In the MSSM, the Higgs self-coupling is suppressed relative to the SM value. Such a suppression was found to be rather weak and the ratio XhMhShSM/XShMhh is above 0.97 due to the tightly constrained parameter space, cf. Figs. 1 and 2;

In the NMSSM with X < 0.7, we consider the case that the SM-like Higgs boson mass is less than twice of mh1, so that h2 will not decay into a pair of hi. We found that the Higgs self-coupling was found to be likely suppressed and the ra-

tio À

NMSSM SM hhh

/ÀhM can be as low as 0.1 due to the large mixing

between singlet and doublet Higgs bosons, cf. Fig. 5. In that case, the coupling of the SM-like Higgs boson (h2) to W and Z bosons and top quark pairs are all suppressed as compared to the SM prediction. On the other hand, its couplings to loop-induced processes, such as photon pairs or gluon pairs, can be enhanced, cf. Fig. 6. Given the limited sensitivity of measuring the Higgs boson self-couplings, we anticipate that the precision measurement of Higgs couplings to gauge bosons and fermions could test this scenario at the LHC and future colliders prior to the direct detection of triple or quartic Higgs couplings;

• In the NMSSM with k > 0.7 (also called k-SUSY), the Higgs self-coupling can be greatly suppressed or enhanced relative to the SM value (the ratio kNMhSSM/kshMh can vary from -1.1 to 1.9), cf. Fig. 7, when h1 is taken as the SM-like Higgs boson. Its coupling to W and Z bosons are always suppressed as compared to the SM predictions. On the contrary, its couplings to tau pairs can be either enhanced or suppressed relative to the SM value, cf. Fig. 9. When mh2 > 2mh1, it is possible to observe a new resonance production in the di-Higgs boson channel at the LHC. While the couplings of h2 to W and Z bosons are always suppressed, its coupling to tau pair can deviate largely from the SM value, depending on the mass of h2, cf. Fig. 8.

Since the NMSSM can give rather different values (compared with the SM) for the trilinear self-couplings of the SM-like Higgs boson, the future collider experiments like the high luminosity LHC or ILC can probe NMSSM through measuring the Higgs self-couplings.

Acknowledgements

Lei Wu thanks Roman Nevzorov, Ulrich Ellwanger, Archil Kobakhidze and Michael Schmidt for very helpful discussions. This work was partly supported by the Australian Research Council, by the CAS Center for Excellence in Particle Physics (CCEPP), by the National Natural Science Foundation of China (NNSFC) under grants Nos. 11305049, 11275057, 11405047, 11275245, 10821504 and 11135003, by Specialized Research Fund for the Doctoral Program of Higher Education under Grant No. 20134104120002, and by the U.S. National Science Foundation under Grant No. PHY-1417326.

References

[1] G. Aad, et al., ATLAS Collaboration, Phys. Lett. B 710 (2012) 49.

[2] S. Chatrachyan, et al., CMS Collaboration, Phys. Lett. B 710 (2012) 26.

[3] For recent reviews, see, e.g., S. Dawson, et al., arXiv:1310.8361 [hep-ex];

C. Englert, et al., arXiv:1403.7191 [hep-ph].

[4] See, e.g., M. Bicer, et al., TLEP Design Study Working Group Collaboration, J. High Energy Phys. 1401 (2014) 164, arXiv:1308.6176 [hep-ex];

D.M. Asner, et al., arXiv:1310.0763 [hep-ph].

[5] S. Kanemura, Y. Okada, E. Senaha, C.-P. Yuan, Phys. Rev. D 70 (2004) 115002, arXiv:hep-ph/0408364;

K.G. Chetyrkin, M.F. Zoller, J. High Energy Phys. 1206 (2012) 033, arXiv: 1205.2892 [hep-ph];

K.G. Chetyrkin, M.F. Zoller, J. High Energy Phys. 1304 (2013) 091, arXiv: 1303.2890 [hep-ph];

A.V. Bednyakov, A.F. Pikelner, V.N. Velizhanin, Nucl. Phys. B 875 (2013) 552, arXiv:1303.4364.

[6] B.A. Kniehl, M. Spira, Z. Phys. C 69 (1995) 77, arXiv:hep-ph/9505225;

S. Dawson, S. Dittmaier, M. Spira, Acta Phys. Pol. B 29 (1998) 2875, arXiv:hep-ph/9806304;

S. Dawson, C. Kao, Y. Wang, P. Williams, Phys. Rev. D 75 (2007) 013007, arXiv:hep-ph/0610284;

D.Y. Shao, C.S. Li, H.T. Li, J. Wang, J. High Energy Phys. 1307 (2013) 169, arXiv:1301.1245 [hep-ph];

J. Grigo, J. Hoff, K. Melnikov, M. Steinhauser, Nucl. Phys. B 875 (2013) 1, arXiv:1305.7340 [hep-ph];

D. de Florian, J. Mazzitelli, Phys. Rev. Lett. 111 (2013) 201801, arXiv:1309.6594 [hep-ph];

L.S. Ling, et al., Phys. Rev. D 89 ( 2014 ) 073001, arXiv:1401.7754 [hep-ph]; X. Li, M.B. Voloshin, Phys. Rev. D 89 (2014) 013012, arXiv:1311.5156 [hep-ph]; R. Frederix, et al., Phys. Lett. B 732 ( 2014) 142, arXiv:1401.7340 [hep-ph]; J. Grigo, K. Melnikov, M. Steinhauser, arXiv:1408.2422 [hep-ph]; S. Dawson, A. Ismail, I. Low, arXiv:1504.05596 [hep-ph].

[7] S. Dawson, S. Dittmaier, M. Spira, Phys. Rev. D 58 (1998) 115012, arXiv:hep-ph/ 9805244;

T. Plehn, M. Spira, P.M. Zerwas, Nucl. Phys. B 479 (1996) 46, arXiv:hep-ph/ 9603205;

S. Dawson, C. Kao, Y. Wang, Phys. Rev. D 77 (2008) 113005, arXiv:0710.4331 [hep-ph];

N.D. Christensen, T. Han, T. Li, Phys. Rev. D 86 (2012) 074003, arXiv:1206.5816 [hep-ph];

J. Cao, et al., J. High Energy Phys. 1304 (2013) 134, arXiv:1301.6437 [hep-ph]; N. Liu, L. Wu, P.W. Wu, J.M. Yang, J. High Energy Phys. 1301 (2013) 161, arXiv:1208.3413 [hep-ph];

U. Ellwanger, J. High Energy Phys. 1308 (2013) 077, arXiv:1306.5541 [hep-ph]; C. Han, et al., J. High Energy Phys. 1404 (2014) 003, arXiv:1307.3790 [hep-ph]; J. Liu, X.P. Wang, S.h. Zhu, arXiv:1310.3634 [hep-ph];

B. Bhattacherjee, A. Choudhury, arXiv:1407.6866 [hep-ph];

N. Liu, S. Hu, B. Yang, J. Han, J. High Energy Phys. 1501 (2015) 008, arXiv: 1408.4191 [hep-ph];

C.Y. Chen, S. Dawson, I.M. Lewis, Phys. Rev. D 91 (2015) 035015, arXiv: 1410.5488 [hep-ph];

V. Martin-Lozano, J.M. Moreno, C.B. Park, arXiv:1501.03799 [hep-ph].

[8] D.E. Ferreira de Lima, A. Papaefstathiou, M. Spannowsky, J. High Energy Phys. 1408 (2014) 030, arXiv:1404.7139 [hep-ph];

D. Wardrope, et al., arXiv:1410.2794 [hep-ph].

[9] U. Baur, T. Plehn, D.L Rainwater, Phys. Rev. D 67 (2003) 033003, arXiv:hep-ph/ 0211224;

U. Baur, T. Plehn, D.L. Rainwater, Phys. Rev. D 69 (2004) 053004, arXiv:hep-ph/ 0310056;

J. Baglio, et al., J. High Energy Phys. 1304 (2013) 151, arXiv:1212.5581 [hep-ph].

[10] M.J. Dolan, C. Englert, M. Spannowsky, J. High Energy Phys. 1210 (2012) 112, arXiv:1206.5001 [hep-ph];

A. Papaefstathiou, L.L. Yang, J. Zurita, Phys. Rev. D 87 (2013) 011301, arXiv:1209.1489 [hep-ph];

F. Goertz, A. Papaefstathiou, L.L. Yang, J. Zurita, J. High Energy Phys. 1306 (2013) 016, arXiv:1301.3492 [hep-ph];

M. Gouzevitch, et al., J. High Energy Phys. 1307 (2013) 148, arXiv:1303.6636 [hep-ph];

A.J. Barr, M.J. Dolan, C. Englert, M. Spannowsky, Phys. Lett. B 728 (2014) 308, arXiv:1309.6318 [hep-ph];

M.J. Dolan, C. Englert, N. Greiner, M. Spannowsky, Phys. Rev. Lett. 112 (2014) 101802, arXiv:1310.1084 [hep-ph];

Q. Li, Q.S. Yan, X. Zhao, Phys. Rev. D 89 (2014) 033015, arXiv:1312.3830 [hep-ph];

P. Maierhöfer, A. Papaefstathiou, J. High Energy Phys. 1403 (2014) 126, arXiv: 1401.0007 [hep-ph];

Q. Li, Z. Li, Q.S. Yan, X. Zhao, arXiv:1503.07611 [hep-ph]; A. Papaefstathiou, arXiv:1504.04621 [hep-ph].

[11] A. Efrati, Y. Nir, arXiv:1401.0935 [hep-ph];

V. Barger, L.L. Everett, C.B. Jackson, G. Shaughnessy, Phys. Lett. B 728 (2014) 433, arXiv:1311.2931 [hep-ph];

N. Haba, K. Kaneta, Y. Mimura, E. Tsedenbaljir, Phys. Rev. D 89 (2014) 015018, arXiv:1311.0067 [hep-ph];

P. Osland, P.N. Pandita, Phys. Rev. D 59 (1999) 055013, arXiv:hep-ph/9806351.

[12] R.S. Gupta, H. Rzehak, J.D. Wells, Phys. Rev. D 88 (2013) 055024, arXiv: 1305.6397 [hep-ph].

[13] R. Barbieri, et al., Phys. Rev. D 87 (2013) 115018, arXiv:1304.3670 [hep-ph].

[14] V.D. Barger, M.S. Berger, A.L Stange, R.J.N. Phillips, Phys. Rev. D 45 (1992) 4128.

[15] M.S. Carena, J.R. Espinosa, M. Quiros, C.E.M. Wagner, Phys. Lett. B 355 (1995) 209, arXiv:hep-ph/9504316;

M.S. Carena, M. Quiros, C.E.M. Wagner, Nucl. Phys. B 461 (1996) 407, arXiv: hep-ph/9508343;

M.S. Carena, et al., Nucl. Phys. B 580 (2000) 29, arXiv:hep-ph/0001002.

[16] J.R. Ellis, G. Ridolfi, F. Zwirner, Phys. Lett. B 262 (1991) 477; J.R. Ellis, G. Ridolfi, F. Zwirner, Phys. Lett. B 257 (1991) 83.

[17] R.J. Zhang, Phys. Lett. B 447 (1999) 89, arXiv:hep-ph/9808299;

J.R. Espinosa, R.J. Zhang, J. High Energy Phys. 0003 (2000) 026, arXiv:hep-ph/ 9912236;

J.R. Espinosa, R.J. Zhang, Nucl. Phys. B 586 (2000) 3, arXiv:hep-ph/0003246.

[18] R. Hempfling, A.H. Hoang, Phys. Lett. B 331 (1994) 99, arXiv:hep-ph/9401219;

H.E. Haber, R. Hempfling, Phys. Rev. D 48 (1993) 4280, arXiv:hep-ph/9307201.

[19] P.N. Pandita, Phys. Lett. B 318 (1993) 338; P.N. Pandita, Z. Phys. C 59 (1993) 575.

[20] T. Elliott, S.F. King, P.L. White, Phys. Rev. D 49 (1994) 2435, arXiv:hep-ph/ 9308309.

[21] U. Ellwanger, C. Hugonie, Eur. Phys. J. C 25 (2002) 297, arXiv:hep-ph/9909260.

[22] K. Funakubo, S. Tao, Prog. Theor. Phys. 113 (2005) 821, arXiv:hep-ph/0409294.

[23] W. Hollik, S. Penaranda, Eur. Phys. J. C 23 (2002) 163, arXiv:hep-ph/0108245.

[24] A. Dobado, M.J. Herrero, W. Hollik, S. Penaranda, Phys. Rev. D 66 (2002) 095016, arXiv:hep-ph/0208014.

[25] D.T. Nhung, M. Mühlleitner, J. Streicher, K. Walz, J. High Energy Phys. 1311 (2013) 181, arXiv:1306.3926 [hep-ph].

[26] M. Brucherseifer, R. Gavin, M. Spira, arXiv:1309.3140 [hep-ph].

[27] V. Khachatryan, et al., CMS Collaboration, J. High Energy Phys. 1410 (2014) 160, arXiv:1408.3316 [hep-ex].

[28] ATLAS Collaboration, ATLAS-CONF-2014-049.

[29] ATLAS Collaboration, ATLAS-CONF-2013-090.

[30] V. Khachatryan, et al., CMS Collaboration, LHCb Collaboration, arXiv:1411.4413 [hep-ex].

[31] M. Papucci, J.T. Ruderman, A. Weiler, J. High Energy Phys. 1209 (2012) 035, arXiv:1110.6926 [hep-ph];

L.J. Hall, D. Pinner, J.T. Ruderman, J. High Energy Phys. 1204 (2012) 131, arXiv:1112.2703 [hep-ph];

J. Cao, et al., J. High Energy Phys. 1211 (2012) 039, arXiv:1206.3865 [hep-ph]; C. Han, et al., J. High Energy Phys. 1310 (2013) 216, arXiv:1308.5307 [hep-ph]; C. Han, et al., J. High Energy Phys. 1402 (2014) 049, arXiv:1310.4274 [hep-ph]; C. Han, D. Kim, S. Munir, M. Park, arXiv:1502.03734 [hep-ph].

[32] A. Arbey, M. Battaglia, A. Djouadi, F. Mahmoudi, J. High Energy Phys. 1209 (2012) 107, arXiv:1207.1348 [hep-ph];

A. Arbey, M. Battaglia, A. Djouadi, F. Mahmoudi, Phys. Lett. B 720 (2013) 153, arXiv:1211.4004 [hep-ph].

[33] For a review of NMSSM, see, e.g., U. Ellwanger, C. Hugonie, A.M. Teixeira, Phys. Rep. 496 (2010) 1;

M. Maniatis, Int. J. Mod. Phys. A 25 (2010) 3505; S.F. King, P.L. White, Phys. Rev. D 52 (1995) 4183.

[34] J. Cao, et al., J. High Energy Phys. 1203 (2012) 086, arXiv:1202.5821 [hep-ph]; J. Cao, et al., J. High Energy Phys. 1210 (2012) 079, arXiv:1207.3698 [hep-ph].

[35] D.J. Miller, R. Nevzorov, P.M. Zerwas, Nucl. Phys. B 681 (2004) 3, arXiv:hep-ph/ 0304049;

R. Nevzorov, D.J. Miller, arXiv:hep-ph/0411275.

[36] U. Ellwanger, C. Hugonie, Mod. Phys. Lett. A 22 (2007) 1581, arXiv:hep-ph/ 0612133.

[37] K. Agashe, Y. Cui, R. Franceschini, J. High Energy Phys. 1302 (2013) 031, arXiv:1209.2115 [hep-ph].

[38] J. Cao, et al., J. High Energy Phys. 1311 (2013) 018, arXiv:1309.4939 [hep-ph].

[39] D. Curtin, R. Essig, Y.M. Zhong, arXiv:1412.4779 [hep-ph].

[40] K. Betre, S.E. Hedri, D.G.E. Walker, arXiv:1407.0395 [hep-ph].

[41] J. Cao, J.M. Yang, Phys. Rev. D 78 (2008) 115001, arXiv:0810.0989 [hep-ph].

[42] J.L Feng, P. Kant, S. Profumo, D. Sanford, Phys. Rev. Lett. 111 (2013) 131802, arXiv:1306.2318 [hep-ph];

P. Kant, R.V. Harlander, L Mihaila, M. Steinhauser, J. High Energy Phys. 1008 (2010) 104, arXiv:1005.5709 [hep-ph];

R.V. Harlander, P. Kant, L. Mihaila, M. Steinhauser, Phys. Rev. Lett. 100 (2008) 191602, arXiv:0803.0672 [hep-ph];

S.P. Martin, Phys. Rev. D 75 (2007) 055005, arXiv:hep-ph/0701051.

[43] J. Beringer, et al., Particle Data Group, Phys. Rev. D 86 (2012) 010001.

[44] U. Ellwanger, J.F. Gunion, C. Hugonie, J. High Energy Phys. 0502 (2005) 006; U. Ellwanger, C. Hugonie, Comput. Phys. Commun. 175 (2006) 290;

G. Belanger, et al., J. Cosmol. Astropart. Phys. 0509 (2005) 001.

[45] S. Heinemeyer, W. Hollik, G. Weiglein, Comput. Phys. Commun. 124 (2000) 76; S. Heinemeyer, W. Hollik, G. Weiglein, Eur. Phys. J. C 9 (1999) 343.

[46] B.C. Allanach, Comput. Phys. Commun. 143 (2002) 305.

[47] A. Djouadi, J.L. Kneur, G. Moultaka, Comput. Phys. Commun. 176 (2007) 426, arXiv:hep-ph/0211331.

[48] P. Bechtle, et al., Comput. Phys. Commun. 182 (2011) 2605; P. Bechtle, et al., Comput. Phys. Commun. 181 (2010) 138.

[49] P. Bechtle, et al., Eur. Phys. J. C 74 (2014) 2711, arXiv:1305.1933 [hep-ph];

P. Bechtle, et al., Comput. Phys. Commun. 181 (2010) 138, arXiv:0811.4169 [hep-ph].

[50] J. Cao, J.M. Yang, J. High Energy Phys. 0812 (2008) 006, arXiv:0810.0751 [hep-ph].

[51] P.A.R. Ade, et al., Planck Collaboration, arXiv:1303.5076 [astro-ph.CO].

[52] D.S. Akerib, et al., LUX Collaboration, arXiv:1310.8214 [astro-ph.CO].

[53] B. Bhattacherjee, A. Chakraborty, A. Choudhury, arXiv:1504.04308 [hep-ph].

[54] M. Carena, I. Low, N.R. Shah, C.E.M. Wagner, J. High Energy Phys. 1404 (2014) 015, arXiv:1310.2248 [hep-ph];

M. Carena, et al., Phys. Rev. D 91 (3) (2015) 035003, arXiv:1410.4969 [hep-ph].

[55] N. Craig, J. Galloway, S. Thomas, arXiv:1305.2424 [hep-ph].

[56] H.E. Haber, arXiv:1401.0152 [hep-ph].

[57] S. Dawson, et al., arXiv:1310.8361 [hep-ex].

[58] T. Gherghetta, B. von Harling, A.D. Medina, M.A. Schmidt, J. High Energy Phys. 1404 (2014) 180, arXiv:1401.8291 [hep-ph];

S.F. King, M. Muhlleitner, R. Nevzorov, Nucl. Phys. B 860 (2012) 207, arXiv:1201.2671 [hep-ph];

J.F. Gunion, Y. Jiang, S. Kraml, Phys. Lett. B 710 (2012) 454, arXiv:1201.0982 [hep-ph];

D.A. Vasquez, et al., Phys. Rev. D 86 (2012) 035023, arXiv:1203.3446 [hep-ph]; U. Ellwanger, C. Hugonie, Adv. High Energy Phys. 2012 (2012) 625389, arXiv: 1203.5048 [hep-ph];

G.G. Ross, K. Schmidt-Hoberg, F. Staub, J. High Energy Phys. 1208 (2012) 074, arXiv:1205.1509 [hep-ph].

[59] J. Cao, et al., J. High Energy Phys. 1412 (2014) 026, arXiv:1409.8431 [hep-ph].

[60] S. Chang, C. Kilic, R. Mahbubani, Phys. Rev. D 71 (2005) 015003, arXiv:hep-ph/ 0405267;

A. Birkedal, Z. Chacko, Y. Nomura, Phys. Rev. D 71 (2005) 015006, arXiv:hep-ph/ 0408329;

A. Delgado, T.M. Tait, J. High Energy Phys. 0507 (2005) 023, arXiv:hep-ph/ 0504224;

T. Gherghetta, B. von Harling, N. Setzer, J. High Energy Phys. 1107 (2011) 011, arXiv:1104.3171 [hep-ph];

N. Craig, D. Stolarski, J. Thaler, J. High Energy Phys. 1111 (2011) 145, arXiv: 1106.2164 [hep-ph];

C. Csaki, Y. Shirman, J. Terning, Phys. Rev. D 84 (2011) 095011, arXiv:1106.3074 [hep-ph];

E. Hardy, J. March-Russell, J. Unwin, J. High Energy Phys. 1210 (2012) 072, arXiv:1207.1435 [hep-ph].

[61] N.D. Christensen, T. Han, Z. Liu, S. Su, J. High Energy Phys. 1308 (2013) 019, arXiv:1303.2113 [hep-ph].

[62] V. Barger, et al., Phys. Rev. Lett. 114 (1) (2015) 011801, arXiv:1408.0003 [hep-ph].