# Extended gauge mediation in the NMSSM with displaced LHC signals

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## Abstract

We analyze models of extended gauge Mediation in the context of the NMSSM, concentrating on supersymmetric spectra with light gluinos, low fine-tuning and decays of the lightest neutralino leading to displaced vertices. While the minimal scenario has rather heavy gluinos as a result of restrictions from the Higgs sector, we propose two new models in which the gluino can be as light as allowed by direct searches at the LHC, with a mass of about \(1.7 \, \mathrm{TeV}\) and \(2.0 \, \mathrm{TeV}\), respectively. Both models have a tuning of a few permille, and lead to an interesting phenomenology due to a light singlet sector. A singlet state at around 98 GeV can account for the LEP excess, while the singlino has a mass of the order of 100 GeV and decays to b-jets and the gravitino, with decay lengths of a few cm.

## 1 Introduction

Gauge mediated supersymmetry breaking (GMSB) is one of the most elegant ways to explain the absence of sizable contributions to flavour violating processes in supersymmetric (SUSY) models. However, its simplest realizations are inconsistent with the measured Higgs mass of 125 GeV, unless one is willing to accept a very heavy (and thus unnatural) SUSY spectrum. In general there are two ways to make GMSB viable with sparticles light enough to be in the LHC reach. The first option to boost the Higgs mass is to maximize the loop corrections with sizable stop mixing, which requires direct Higgs-messenger couplings [1, 2, 3, 4, 5, 6, 7, 8, 9, 10, 11, 12, 13, 14, 15, 16, 17, 18, 19, 20, 21]. The second (less explored) option is to introduce additional tree-level contributions to the Higgs mass. Such corrections may originate from the mixing of the Higgs with a lighter singlet [22], and can be realized in a simple model proposed by Delgado, Giudice and Slavich (DGS) [23] that combines the NMSSM and GMSB with direct singlet-messenger couplings. Indeed it has been shown in Ref. [24] that the most interesting region in parameter space features a light SUSY spectrum and a singlet around \(90\ \div 100\ \hbox {GeV}\), which gives a sizable tree-level contribution to the SM-like Higgs mass through mixing. Besides this “push-up” of the Higgs mass, the general framework of NMSSM+GMSB with a light singlet has other advantages. First, it provides a natural solution to the \(\mu \)-\(B_\mu \) problem [23], as \(\mu \) and \(B_\mu \) are generated dynamically through the vacuum expectation value (VEV) of the singlet. Second, the Next-to-Lightest SUSY particle (NLSP) is typically the singlino, whose decay into the gravitino is suppressed, leading to novel displaced signatures at colliders [25].

In the present paper, we focus on \(\hbox {GMSB} + \hbox {NMSSM}\) models with direct matter-messenger couplings, with a special emphasis on displaced signatures. This is motivated by recent LHC results for heavy Higgs searches in the \(\tau \tau \) channel [26], which has excluded the most interesting part of the parameter space of the DGS model. We investigate two simple extensions of the DGS model leading to a relatively light sparticle spectrum, which can be probed in the second run of the LHC, in particular associated with displaced decay signatures.

The rest of the article is organized as follows: In Sect. 2 we analyse the general features of SUSY models with light singlets. In Sect. 3 we review the DGS model and investigate the impact of recent LHC results on its parameter space. In Sects. 4 and 5 we introduce two new models with singlet-messenger couplings, and summarize and conclude in Sect. 6. In an Appendix we provide complete expressions for soft terms in the respective models.

## 2 EWSB in the NMSSM with a light singlet

*v*is the electroweak scale, in which one finds

*lighter*singlet-like Higgs, thus allowing to lower the overall scale of the SUSY spectrum that drives the radiative corrections to the Higgs mass.

In the following we revisit this model (DGS) in the light of updated experimental constraints, and compare it to the phenomenology of two similar models that feature additional singlet-messenger couplings. We are particularly interested in SUSY spectra with experimental signatures that may be probed at the LHC using displaced vertices, as studied in Ref. [25].

*H*/

*A*decaying to \(\tau \tau \), because the cross-section for

*H*/

*A*production grows with \( \tan ^2 \beta \). Since this constraint turns out so important, it is instructive to discuss the origin of large \(\tan \beta \) in the push-up region of NMSSM models with gauge Mediation. Neglecting \(m_{H_d}^2\), which is usually a good approximation in the models under consideration, the expression for \(\tan \beta \) is relatively simple:

^{1}, \(A_\kappa \) must be negative to avoid tachyons in the singlet sector. In the limit \(w\gg 1\), corresponding to the case where EWSB is driven by a large negative \(m_S^2\), one finds indeed large values of \(\tan \beta \)

*w*the value of \(\tan \beta \) slightly decreases. In the limit \(w\approx 1/3\) one finds

*Z*-boson mass that is convenient to assess the fine-tuning. In the large \(\tan \beta \) limit one has

*z*defined in Eq. (3). For the fine-tuning \(\varDelta \) we use the Barbieri-Giudice measure [28]

We conclude this section with a brief comment of the potential tuning related to the “push-up” contribution to the SM-like Higgs mass, which can be relevant if \(\lambda \) is sizable [29, 30]. In our case however, this source of tuning is absent, since \(\lambda \ll 1\) (as we are going to see in the next sections), so that the contribution from mixing \(\delta m^2_\mathrm{mix}\) is small, (few GeV)\(^2\), as compared to the total Higgs mass.

## 3 The DGS model

*S*), in addition to two copies of messengers in \(\mathbf{5} + \mathbf{\overline{5}}\) representations of SU(5). The superpotential is given by the NMSSM (see Appendix for our conventions), the spurion-messenger couplings of ordinary gauge mediation and new singlet-messenger couplings. Apart from the NMSSM part we have

*X*denotes the SUSY breaking spurion that takes the VEV \(\langle X \rangle = M + F \theta ^2\). This superpotential gives rise to soft SUSY breaking terms that can be found in the Appendix. These are determined by six parameters: the messenger scale

*M*, the NMSSM couplings \(\lambda \) and \(\kappa \), the DGS couplings \(\xi _D\) and \(\xi _T\) and the effective scale of soft SUSY breaking terms \(\tilde{m} \equiv 1/(16 \pi ^2) F/M\). One of these parameters (following DGS we choose \(\kappa \)) can be eliminated by requiring correct EWSB. We also impose a unification condition for \(\xi _D\) and \(\xi _T\) that allows to eliminate one additional parameter,

In order to assess this issue, we have updated the analysis of the DGS model in Ref. [24] using the latest LHC constraints. For this analysis we have used the public code NMSSMTools [32, 33], which computes the SUSY and Higgs spectrum and checks the latest LHC constraints in the Higgs sector (LHC constraints on SUSY sector will be dealt with later with CheckMATE2). We have performed large MCMC scans of the parameter space of the DGS model and sorted the results in a 2D histogram in the plane of the gluino mass vs. the decay length of the singlino NLSP. In each bin of this histogram, we have kept the point in parameter space minimising the fine-tuning as defined in Eq. (11). In Fig. 1 we present a map of fine-tuning in the plane of the gluino mass and the decay length of the singlino NLSP. We see that for NLSP decay lengths corresponding to a displaced vertex, the gluino mass is pushed far beyond 3 TeV. Thus, the DGS model does not predict any displaced signatures that could be observed at the LHC. We also note that even for larger NLSP decay length, for which the NLSP is stable from the LHC perspective, the gluino must be heavy and may be beyond the LHC discovery reach. Numerically, we find a lower bound on the gluino mass of \(1.8 \, \mathrm{TeV}\), and a lower bound on the tuning of \(\varDelta \ge 600 \).

These negative conclusions can be traced back to recent heavy Higgs searches in the \(\tau \tau \) channel [26], which exclude previously viable points with light gluinos. This happens because successful EWSB in the DGS model with a light singlet requires rather large values of \(\tan \beta \gtrsim 30\), which pushes the heavy MSSM-like Higgs bosons to values above 1.3 TeV [26], and thus requires larger SUSY scales.

## 4 The U model

In Fig. 2 we present a map of fine-tuning in the plane of the gluino mass and the decay length of the singlino NLSP, obtained analogously to Fig. 1. One can clearly distinguish two different regions here, in the upper part the “DGS-like” region, that is characterised by a large NLSP decay length \(c \tau _{\tilde{N}_1} \gtrsim 100 \, \mathrm{cm}\), small fine-tuning \(\varDelta \lesssim 10^3\), a light singlet spectrum (\(m_{a_1} \approx 30 \div 40\ \hbox {GeV}\), \(m_{h1} \approx 90\ \hbox {GeV}\), \(m_{\tilde{S}} \approx 100\ \hbox {GeV}\)) and an essentially constant input value \(\lambda _{S_d} \sim 10^{-2}\). Representative for the DGS-like region are the benchmark points P1 and P2 in Table 1. A closer look reveals that this region actually falls into two sub-regions, which can be separated by the value of the gluino mass as visible in Fig. 2. For gluino masses above 1.8 TeV, the value of \(|\lambda _t|\) is essentially constant, \(\sim 0.3\), while it increases up to \(\sim 0.7\) towards lighter masses. Moreover, these parts are distinguished by the value of \(\ tan \beta \), which is about 10 in the left part and about 20 in the heavy gluino part. The latter is represented by P1 while P2 exemplifies the light gluino part of the DGS region.

The other region with smaller NLSP decay lengths \(c \tau _{\tilde{N}_1} \lesssim 100 \, \mathrm{cm}\) is represented by benchmark P3 in Table 1. This region features much larger tuning \(\varDelta \gg 10^3\), essentially constant \(\tan \beta \approx 10\), a heavier singlet spectrum (\(m_{a1}, m_{\tilde{N}_1} \gtrsim 200\ \hbox {GeV}\)), large constant values of \(|\lambda _t| \approx 0.7\) and \(\lambda _{S_d} \approx 0.2\) and a potentially lighter gluino mass compared to the DGS-like region. From Fig. 2 one can see that a singlino decay length \(\mathcal {O}(1) \, \mathrm{cm}\) is possible for a gluino as light as about 1 TeV, without being in conflict with Higgs sector constraints. Nevertheless, such a light gluino might be already excluded by direct searches at the LHC.

We have therefore taken into account the LHC limits from direct SUSY searches with CheckMATE2 [34]. To briefly summarise the workflow, CheckMATE2 uses Pythia8 [35] to generate all accessible \(2\rightarrow 2\) processes followed by a detector simulation with Delphes3 [36]. Variables and cuts used in experimental analyses are then implemented as closely as possible to “recast” the analysis, and the expected number of signal events that pass the cuts are validated against published benchmarks and cut flows. This validated analysis can then be used to test New Physics models against published upper limits. In the presence of multiple signal regions that may potentially be sensitive to model predictions, CheckMATE2 selects only the most sensitive region with respect to the expected background.

Benchmarks consistent with all experimental constraints, including LHC direct search limits. P1–P3 are points in the U model, while P4–P6 belong to the DGSU model. All points have reduced SM-like Higgs signal strengths of about 0.84, corresponding to a Higgs-singlet mixing angle of \(\cos \theta \approx 0.92\), while the signal strengths of the singlet-like state are about 0.16. All soft masses are at the SUSY scale. We note that Higgs decays with \(a_1\) in final states are strongly suppressed due to small \(\lambda \)

P1 | P2 | P3 | P4 | P5 | P6 | |
---|---|---|---|---|---|---|

\(\tilde{m}\) [TeV] | 1.7 | 1.5 | 1.5 | 0.87 | 1.0 | 1.0 |

| \(2.8 \times 10^{6}\) | \(3.1 \times 10^{6}\) | \(2.5 \times 10^{6}\) | \(5.6 \times 10^{6}\) | \(5.1 \times 10^{6}\) | \(1.6 \times 10^{6}\) |

\(\lambda \) | \(4.6 \times 10^{-3}\) | \(4.4 \times 10^{-3}\) | \( 1.1 \times 10^{-3}\) | \(4.9 \times 10^{-3}\) | \(5.4 \times 10^{-3}\) | \(2.5 \times 10^{-3}\) |

\(\kappa \) | \(1.4 \times 10^{-4}\) | \(1.2 \times 10^{-4}\) | \( 4.3 \times 10^{-5}\) | \(1.5 \times 10^{-4}\) | \(2.1 \times 10^{-4}\) | \(6.5 \times 10^{-5}\) |

\(\lambda _t\) | \(-\,0.33\) | \(-\,0.48 \) | \(-\,0.73\) | \(-\,0.64 \) | \(-\,0.38 \) | 0.76 |

\(\lambda _{S_d}\) | 0.022 | 0.028 | 0.17 | – | – | – |

\(\xi \) | – | – | – | 0.012 | 0.010 | 0.010 |

\(\tan \beta \) | 18 | 11 | 10 | 9.1 | 17 | 8.7 |

\(m_{\tilde{g}}\) [TeV] | 2.0 | 1.7 | 1.8 | 2.0 | 2.3 | 2.2 |

\(m_{\tilde{d}_R}\) [TeV] | 2.6 | 2.2 | 2.3 | 2.0 | 2.4 | 2.3 |

\(m_{\tilde{t}_1}\) [TeV] | 2.1 | 1.7 | 2.2 | 1.8 | 2.0 | 2.2 |

\(m_{\tilde{N}_1}\) [GeV] | 95 | 96 | 200 | 96 | 97 | 106 |

\(m_{\tilde{N}_2}\) [GeV] | 370 | 320 | 330 | 380 | 440 | 430 |

\(m_{a_1}\) [GeV] | 26 | 32 | 290 | 26 | 24 | 26 |

\(m_{a_2}\) [TeV] | 1.7 | 1.9 | 2.7 | 1.6 | 1.4 | 2.1 |

\(m_{h_1}\) [GeV] | 89 | 89 | 110 | 89 | 91 | 101 |

\(m_{\mu L}\) [GeV] | 960 | 830 | 820 | 710 | 840 | 790 |

\(m_{\mu R}\) [GeV] | 480 | 430 | 520 | 390 | 420 | 450 |

\(m_{\chi _1^\pm }\) [GeV] | 720 | 620 | 640 | 720 | 840 | 830 |

\(m_{H_u}^2\) [TeV\(^2\)] | \(-\,2.2\) | \(-\,2.8\) | \(-6.8\) | \(-\,2.2\) | \(-\,1.5\) | \(-\,3.9\) |

\(m_{H_d}^2\) [TeV\(^2\)] | 0.75 | 0.62 | 0.59 | 0.47 | 0.58 | 0.58 |

\(m_{S}^2\) [GeV\(^2\)] | \(-\,4.3 \times 10^3\) | \(-\,4.3 \times 10^3\) | \(7.8 \times 10^3\) | \(-\,4.3 \times 10^3\) | \(-\,4.5 \times 10^3\) | \(-\,5.3 \times 10^3\) |

\(A_\lambda \) [GeV] | 64 | 130 | 180 | 150 | 52 | 210 |

\(A_\kappa \) [GeV] | \(-\,4.9\) | \(-\,7.2\) | \(-\,280\) | \(-\,4.8\) | \(-\,3.9\) | \(-\,4.3\) |

\(c \tau _{\tilde{N}_1}\) [cm] | 200 | 200 | 10 | 200 | 200 | 12 |

\(\varDelta \) | 530 | 680 | 37000 | 440 | 310 | 720 |

*w*, which follows from

*w*approaches 1 / 3 for which \(\tan \beta \) is twice as small as in the limit \(w\gg 1\), as explained

^{2}in Sect. 2. Therefore, the combined effect of increased \(m_{a2}\) and decreased \(\tan \beta \) renders the LHC searches for heavy Higgs bosons with \(\tau \tau \) final states essentially insensitive to the U model with large \(\lambda _t\) and light gluinos.

While \(\lambda ^2/\kappa ^2 \sim 10^3\) is essentially constant in both regions, the smallness of \(\lambda _{S_d} \sim 10^{-2}\) in the DGS-like region implies that the second term in Eq. (19) is small, and the tuning is essentially determined by \(\lambda _t^2 \tilde{m}^2\), with a minimal value of \(\varDelta \approx 450\). Instead the other region features large \(\lambda _{S_d} \sim 0.2\), which together with large \(\lambda _t\) leads to a significant enhancement of the tuning with respect to the DGS-like region, by about a factor 100. This estimate explains the large increase in the tuning when crossing between the two different regions in Fig. 2. It also accounts for the approximately constant tuning over the two DGS-like sub-regions, where a decrease in the gluino mass (i.e. \(\tilde{m}\)) is compensated by an increase in \(\lambda _t\), such that the total tuning remains essentially constant, up to \(\mathcal{O}(1)\) factors.

We conclude this section with a discussion of the three benchmark points P1–P3 in Table 1, which represent sample spectra of the U model with a light SUSY spectrum compatible with all LHC constraints, with a singlino decay length roughly below two meters. The point P1 features a tuning of \(\varDelta \approx 500\), with a gluino mass around 2 TeV and NLSP singlino decay length about 2 m. This point represents the DGS-like region in the upper right corner with large \(\tan \beta \). The point P2 has larger \(\lambda _t\approx 0.5\), which allows for a lighter gluino, although the tuning slightly increases as discussed above. The larger \(\lambda _t\) implies smaller \(\tan \beta \approx 11\), while the light singlet spectrum is quite similar to P1, with a NLSP singlino decay length that is still relatively large, \(c \tau _{\tilde{N}_1} \approx 1.9 \, \mathrm{m}\). For both P1 and P2, the singlino NLSP mainly decays to the gravitino and the lightest pseudoscalar \(a_1\) (with mass \(\sim 30\ \hbox {GeV}\)) which in turns decays promptly to \(b \overline{b}\). Characteristic for these benchmarks is a light Higgs state \(h_1\) with mass around 90 GeV, which is mainly a SM singlet with a small doublet admixture corresponding to a mixing angle \(\cos ^2 \theta \approx 0.84\). This state might account for the \(2\sigma \) excess observed at LEP [31, 39] in the \(b\bar{b}\) channel, and could also explain the tentative hint for a light Higgs decaying into diphotons at CMS [40], although the signal strength of the light singlet state in the diphoton channel is about a factor of three smaller than the current central value of the CMS excess.

On the other hand, NLSP decay lengths below \(1 \, \mathrm{m}\) can only be obtained for the price of increased fine-tuning, in the region where \(\lambda _t \approx 0.7\) is constant. This is exemplified by the point P3, which features \(c \tau _{\tilde{N}_1}\approx 10\) cm and a tuning of at least \(\varDelta \approx 10^4\). These points have a heavier Higgs spectrum, and in particular the lightest pseudoscalar is now heavier than 250 GeV, while the NLSP singlino is above 200 GeV. In contrast to P1 and P2, here the singlino mainly decays to gravitino and \(h_1\) (with mass \(\sim 110\ \hbox {GeV}\)), since \(a_1\) is too heavy.

## 5 The DGSU model

^{3}now impose the Higgs-messenger mixing condition (for simplicity at the messenger scale)

*M*, \(\lambda \), \(\kappa \), \(\xi \) and \(\lambda _t\) (the same number as in the U model).

In Fig. 5 we present a map of fine-tuning in the plane of the gluino mass and the decay length of the singlino NLSP, obtained analogously to Figs. 1 and 2. However, comparing to the exclusion limits from direct LHC searches shown in Fig. 6, we see that they are stronger than in the U model and the allowed points can have gluino masses only slightly below 2 TeV. The reason for this is that in the DGSU model there are two messengers (in contrast to one in the U model). Since the minimal gauge mediation contribution to gaugino masses is proportional to the number of messengers *N* while the corresponding contribution to sfermion masses scales as \(\sqrt{N}\), cf. (A.3), this makes sfermions lighter for a given gaugino masses. As a result, the squarks of the first two generations are comparable to the gluino mass and their production cross-section is non-negligible. For the same reason left-handed sleptons of the first two generations can now be lighter than wino, which results in more leptons in the final state (instead of \(\tau \)’s as in the U model). The latter feature of the DGSU model also explains why the constraints for larger NLSP decay lengths are weaker, since the larger decay length is obtained for larger messenger scale, which in turn results in heavier sleptons (as compared to gauginos) due to their stronger renormalization by electroweak gauginos. Nevertheless, a gluino mass of 2 TeV is still viable for a decay length \(\mathcal {O}(1)\) m, while decay lengths roughly between 20 and 100 cm implies a limit for the gluino mass of almost 2.5 TeV. We should also emphasize that this limit is particularly strong not only due to gluino/squark production, but also due to direct production of sleptons and winos, whose mass is correlated with the gluino mass. Therefore also direct searches for direct electroweak production set important constraints [41], besides analyses using jets and missing energy.

Note that for decay lengths of \(\mathcal {O}(10)\) cm, there is a small strip of allowed points (represented by benchmark point P6), which however correspond to larger tuning, cf. Fig. 5. This is a consequence of large values of \(|\lambda _t|\), which also explains the relaxed LHC constraints. For large values of \(|\lambda _t|\), there is a large positive contribution to stop masses at the messenger scale, cf. (A.14), which leads to heavier stop masses at low scales, so that gluino decays to stops are kinematically forbidden.

We notice that the DGSU model shares many features with the DGS model, or rather the DGS-like region of the U model. In particular, all points (represented by benchmarks P4–P6 in Table 1) have a well-defined singlet sector with a singlet-like scalar \(h_1\) around 90–100 GeV, a singlet-like pseudoscalar \(a_1\) around 20–30 GeV and a singlino NLSP between 90–100 GeV. The singlino NLSP decay length can be rather short, of the order of \(\mathcal{O}(10)\) cm, and it decays mainly to gravitino and \(a_1\), which decays promptly to \(b \overline{b}\). The input parameters are essentially constant throughout the whole region, with \(\lambda \sim 10^{-3}\) and \(\xi \sim 10^{-2}\). As in the DGS-like region of the U model one can further distinguish two sub-regions, which are characterised by different values of \(|\lambda _t|\) (that is essentially constant \(\sim 0.4\) for gluino masses above \(\sim \) 2.2 TeV, and below this value starts increasing towards lighter gluino masses, up to \(\sim 0.8\)) and \(\tan \beta \), which is correlated with \(\lambda _t\) similar as in Fig. 4. These two parameters essentially control the mass of the MSSM-like pseudoscalar \(a_2\) and the tuning. The mass of the former grows for larger \(\lambda _t\) (a feature inherited from the U model), and thus is no longer correlated with the gluino mass so that \(H/A\rightarrow \tau \tau \) searches do not constrain this model. Moreover, large values of \(\lambda _t\) lead to a large contribution to the Higgs mass from stop mixing, which implies that the overall SUSY scale can be lowered, and gluinos and stops can be quite light. The DGSU model is thus a perfect realization of the pNMSSM scenario analysed in Ref. [25], and motivates the combined searches using displaced and prompt signatures advocated in that article.

Finally, the DGSU model is also much less fine-tuned than the points with light gluinos in the U model. This can be again understood from the fact that \(\lambda _t\) (which is sizable) dominates the total tuning, and contributes as in Eq. (19) with \(\lambda _{S_d}\) replaced by \(\xi \). Similar to the DGS-like region of the U model, this contribution is small, so that the tuning is controlled by \(\lambda _t^2 \tilde{m}^2\), with a minimal^{4} value of \(\varDelta \approx 300\), which is reached for intermediate values for the gluino mass around 2.3 TeV, where the product of \(\lambda _t\) and \(m_{\tilde{g}}\) is minimal.

## 6 Summary and conclusions

In this article we have analyzed models of extended Gauge Mediation in the context of the NMSSM. The simplest scenario (DGS) requires rather heavy gluinos, which are constrained not by direct SUSY searches but rather a two-fold restriction coming from the Higgs sector. On the one hand, the mass of the SM-like Higgs requires sizable loop corrections, on the other hand direct LHC Higgs searches in the \(\tau \tau \) channel set stringent lower limits on the mass of the heavy Higgses, which in turn is tied to the SUSY scale. We have proposed two new models with singlet/Higgs-messenger couplings (the U model and the DGSU model), which ease these constraints and thus allow for gluinos as light as allowed by direct searches. First, the presence of a direct coupling of stops to the messenger fields generate sizable \(A_t\) at the messenger scale, which in turn allows for much lighter stops (and thus also other sparticles) consistent with the measured SM-like Higgs mass. Second, the same coupling also generates new contributions to the soft Higgs mass, which allows to both increase the MSSM-like Higgs doublet mass and reduce \(\tan \beta \), such that the LHC searches for heavy Higgs are satisfied without raising the overall SUSY scale. To identify the lower bound on the gluino mass in these models, we have recasted the existing LHC searches and found that gluinos can be as light as about \(1.7 \, \mathrm{TeV}\) (U model) and \(2.0 \, \mathrm{TeV}\) (DGSU model). The tuning in both models is rather low, and can be as small as \(2\permille \) (U model) and \(3\permille \) (DGSU model). The phenomenology is quite different in the two models: in the U model there are essentially two distinct regions, one with a DGS-like spectrum featuring a light singlet sector, large singlino decay lengths roughly above a meter (but small enough to see a displaced vertex in the LHC detectors) and low fine-tuning. The other region is characterized by a heavy singlet sector, less displaced singlino decays with \(c \tau _{\tilde{N}_1}\approx 1\div 10\ \hbox {cm}\) and large tuning. The DGSU model combines the most interesting phenomenological features of both regions: light gluinos in the reach of LHC, a light singlet sector with a 98 GeV state (that might account for the LEP excess and improves the fit to the CMS data hinting at a new light state decaying to \(\gamma \gamma \)), and displaced singlino decays into \(b \overline{b} + \hbox {MET}\) with decay lengths as small as a few cm. In Table 1 we have collected benchmark points representative for the relevant parameter regions and the two models.

## Footnotes

- 1.
Also \(\mu < 0\) leads to viable spectra, but we will not consider these scenarios in the following, since the gluino is always quite heavy with a mass above 3.2 TeV.

- 2.
For large \(\lambda _t\), \(\tan \beta \) is suppressed even more due to the RG effect of \(A_t\) which makes \(A_\lambda \) positive at the EW scale and cannot be neglected in Eq. (11). This effect is partially compensated by the fact that \(\lambda _t\) increases \(m_{a2}\) that enters in the numerator of the formula for \(\tan \beta \) in Eq. (11).

- 3.
This is because the singlet scalar mass is now set by \(\xi \sim 10^{-2}\) as in the DGS model, instead of \(\lambda _{S_d}\) as in the U model.

- 4.
This is a factor of a few smaller than the minimal tuning found for a broad class of extended GMSB models in the context of the MSSM [10].

## Notes

### Acknowledgements

The authors acknowledge the support of France-Grilles and the OCEVU Labex (ANR-11-LABX-0060) for providing computing resources on the French National Grid Infrastructure, and support from the French research project Defi InFIniti - AAP 2017. MB and RZ thank the Galileo Galilei Institute for Theoretical Physics and INFN for hospitality and partial support during the completion of this work. MB has been partially supported by the National Science Centre, Poland, under the research grant no. 2017/26/D/ST2/00225. N.D. was supported by the OCEVU Labex (ANR-11-LABX-0060) and the A*MIDEX project (ANR-11-IDEX0001-02) funded by the “Investissements d’Avenir” French government program managed by the ANR.

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