JHEP09(2017)101 Jj )

JHEP09(2017)101 jj ). We jj , and b ¯ Springer )( b b ¯ , b July 21, 2017 ¯ t t : September 4, 2017 searches impose September 21, 2017 : t : . We point out the ), and ( b b ¯ b Received ( or ¯ t t j ) and 4 ), Accepted = Published jj JJ ( J ¯ t )( t JJ Published for SISSA by https://doi.org/10.1007/JHEP09(2017)101 ) decays and ﬁnd their sensivity surpasses b ¯ b ( ¯ t t ) and [email protected] , jj ( ¯ t t . 3 of 13 TeV data. 1 − 1706.07057 The Authors. c Phenomenological Models

We analyze the collider sensitivity for new colored resonances in , [email protected] PRISMA Cluster of ExcellenceJohannes & Gutenberg Mainz University, Institute for55099 Theoretical Mainz, Physics, Germany E-mail: Open Access Article funded by SCOAP Keywords: ArXiv ePrint: propose analysis strategies for the that of existing searchesno when other the decay decays widths are1.5 to TeV present, using tops collective 37 and fb lower light limits jets on are the comparable. resonance If mass can be set at Abstract: final states. While searches inproduction the rate single production is channel model arestrong model-dependent, independent constraints the on and pair the the relevantmissing, existing branching complementary fractions, ( searches where in the mixed decay modes, Malte Buschmann and Felix Yu Collider constraints and newvectors tests of color octet JHEP09(2017)101 ]. 25 – ] also 21 38 – 32 ]. In Randall- 13 – ], the KK gluons 11 20 – 7 ) 16 b ¯ b ] are similarly motivated ( ¯ t t 10 2 , ], massive color octet vectors, 9 , 7 4 – 2 ) and 4 6 jj ( ]. Searches for four tops [ ¯ t 4 t 31 ] offer complementary probes compared 47 – 41 9 – 1 – 7 resonances [ ¯ t t ], most recently constraining colorons with a 100% branching 2 decays of pair-produced resonances. Searches for TeV-scale di- 31 ]. Even so, the colored particle decay patterns and corresponding ] with SM fields propagating in the bulk [ – ¯ t 1 t ] and 26 15 , ], are heavy cousins of the familiar gluon and can decay universally to 40 14 , 1 8 13 39 ]. 49 ]. The non-resonant phenomenology of heavy octet vectors has recently been 48 At the LHC, CMS and ATLAS have searched for color octet vector resonances in the In models with an extended color gauge symmetry [ 3.1 Event selection3.2 strategy Comparison with current searches 2.2 Color octet2.3 vectors from extra Non-universal dimensions couplings2.4 and flavor constraints Collider phenomenology of color octet vectors 2.1 Color octet vectors from extended color gauge groups fraction to light jetsconstrain to the be possible heavierjet than 1.5 resonances TeV [ [ to the pair-production searches,coupling since [ such searches scalediscussed in with [ the individual production Sundrum models [ exhibit flavor-dependent couplings toflavor quarks quark as pairs, a result and of preferentially the localization decay of to the the bulkpaired fermion heavy dijet wavefunction profile channel [ [ Standard Model (SM) quark-anti-quark pairs.by ascribing Axigluons chiral [ projection operatorsfermions to the transforming parent non-trivially gauge under groups,Similar which the necessitates phenomenology extended new occurs gauge in group modelscolor to of octet cancel vectors universal arise extra anomalies. as dimensions, Kaluza-Klein where (KK) the excitations massive of the gluon [ pair production, where leadingcolor charge order and cross mass [ sectionscollider signatures can are be highly calculated model dependent. knowing only the such as colorons [ 1 Introduction Searches for new particles andendeavor new for forces the beyond ATLAS the and Standardsuch CMS Model results experiments (BSM) are at have a the thus critical Large far Hadron Collider come (LHC), up but null. The largest rates come from colored particle 4 Conclusion 3 Collider analyses of the mixed channels, Contents 1 Introduction 2 Theory background JHEP09(2017)101 , η λ to (2.2) (2.1) X transi- , and γ κ s , X λ searches and , t → R ]. The diagonal b gauge group, the d 8 2 , µ a 3 ) and 4 ηX a SU(3) JJ T )( µ × γ 1 , respectively. The Goldstone R JJ 2 ¯ d + R u is , µ a µ 2 2 and SU(3) 1 X X h a 1 are the SU(3) generators, and + gauge group, which imposes the requirement κT . c a 1 2 µ 1 4 h T γ – 2 – R = u 2 s 1 + ¯ g L Q ) mixed decay modes at the LHC and compare with the b ¯ µ a b , we analyze the prospects for discovering color octet vector ( X ¯ t 3 t a λT µ γ ) and L ¯ jj Q , nonzero off-diagonal entries are possible in principle and correspond ( ¯ t t s g are the gauge couplings of SU(3) , we review the theory motivation and collider phenomenology of massive 2 CPT 2 h L ⊃ ], the simplest ansatz is to adopt a flavor-universal coupling structure, evading is the strong coupling constant, and matrices are diagonal but not universal in the quark gauge basis. Moving to the 51 , S 1 ). η g h 50 2.1 In section Given the possibility that the color octet vector has flavor dependent branching frac- , and subgroup is then identified with the SM SU(3) where modes of the complex scalar field become the longitudinal degrees of freedom for the heavy 2.1 Color octetIn vectors models from with extended an colortwo extended gauge parent color groups symmetry, gauge such groups asexpectation a are value SU(3) typically (vev) broken of to a the bifundamental, complex diagonal scalar subgroup field by Σ the [ vacuum κ quark mass basis will thenMaskawa induce (CKM) off-diagonal mixing. entries We proportional willand to first then Cabibbo-Kobayashi- briefly discuss review the models collider ofeq. and massive ( flavor color physics octet phenomenology vectors of the general Lagrangian, to tree-level flavor violation.precision Since flavor these measurements, processes such are astions strongly [ meson constrained mixing by low-energy measurementsthe and most stringest flavor bounds.light In quarks vs. such tops a is scenario, fixed, however,searching and the there in branching is dijet ratio no model vs. for freedom ditop in resonances. the complementarity between Hence, we will focus on the scenario where the where are the flavor-dependent couplings insymmetric the quark by gauge basis. While these matrices must be Massive color octet vector resonancesextensions, arise such in as various different models beyond withsions. the extended Standard In color Model the gauge unbroken groups phasebetween or of quarks models electroweak and with symmetry, a the extra massive general dimen- color interaction octet Lagrangian vector color octet vectors. In section resonances in the current constraints. We conclude in section 2 Theory background tions to quark pairs,duction and rate, because the color mixed octetmotivated. decay vectors signature This have of channel a a is modeleven paired complementary independent offers to ditop superior pair the sensitivity and pro- when existing dijetditops the ( resonance are branching comparable. is fractions of strongly the resonance to dijets and JHEP09(2017)101 ), Y 1 , (2.6) (2.7) (2.3) (2.4) (2.5) gauge U(1) ( 2 , × ) ∼ i 2 1 ), we can q 2 , µ 1 R 2.1 u SU(3) X a ), × T µ 1 , γ ) originate by con- i 1 ¯ q ( 4 2.1 ∼ ... under one SU(3) gauge X 3 L , =1 i ], where left-handed (LH) Q ], we will only focus on the )Σ + 2 a ), 52 , q , R 1 T ) ) and the RH quarks transform b , 9 , , µ R 1 , µa 2 , µ 2 µ 2 4 X ( G θP a 2 3. The corresponding massive color . Explicitly, the covariant derivative ∼ T / θ G θ G i q . ih µ 2 a cot µ 2 Σ , γ h 1 L − + X cos − R a a Q b ¯ L + sin ( − T , we get the SM gluon and coloron fields, T θ c µ µ 1 µ 1 θP µa 1 ¯ qγ – 3 – G tan θ G θ θ G 1 s (tan g SU(3) ih a µ tan − s X → ) is the mixing angle. = cos = sin ) + a g µ 2 2 L µ µ T ∂ b g µ /h µ X 1 , for example, the resulting massive color vector interaction ], all SM quarks transform as 2 ¯ X has non-universal couplings. qγ h ]. This assignment also requires additional matter to cancel s ( a 8 SU(3) , 2 µ 1 g Σ = ( T 3 − µ × X µ )[ γ 1 1 D SU(3) , L ), each with hypercharge b ¯ × 1 1 ( = tan , , but this new matter content can be massive and unobservable at + as before. Although topcolor models are generally motivated by com- θ Y t ∼ µ 2 3 . For example, the topcolor model charges the third generation quarks , X 2 2 /h , a U(1) 1 1 R T d h µ × ) and ( ), = 2 2 is commonly referred as an axigluon in the literature. ¯ tγ SU(3) ( , θ a µ θ , 1 ) under SU(3) × 1 X ( 1 , cot To motivate a non-universal yet diagonal coupling structure in eq. ( In the coloron model [ In this setup, different possibilities for the couplings in eq. ( 1 s ∼ g 3 R with tan posite Higgs scenarios triggeredmotivated by possibility top that quark condensation [ u anomalies, for which a minimaling solution involves as two electroweak ( singlet quarksoctet transform- vector does not havefeatures flavor-changing distinct couplings couplings in to the light quark and gauge heavy basis, generation but quarks: instead where straightforwardly assign different quarkSU(3) flavors to differentdifferently gauge than the representations first under two generations, with and SU(3) colliders. As a result,as if ( the LH quarkswith transform quarks as is ( couplings to the SM quarks as An alternative prescription isand right-handed the (RH) chiral quark color fieldsconstruction are generally model charged requires [ under new different fermions SU(3) to gauge cancel groups. anomalies, notably This SU(3) symmetry. The maintations feature are for assigned universally identicallygauge to coupled symmetry the models commutes same with is gauge the that representation, global which all SM ensures quark flavor flavor thatgroup represen- symmetry. the and singlets under the other. Hence, the coloron has flavor universal, purely vector respectively, where sidering various charge assignments of the quarks in the parent SU(3) octet scalar as thefor dynamical Σ scalar is fields below and after Higgsing SU(3) color octet vector, leaving one real and one pseudoreal color singlet scalar and one real color JHEP09(2017)101 , ], Q c 53 (2.9) (2.8) ], we 51 , , 50 2 s g ]. In order to is fixed by the 2 , RH down-type 11 25 u − KK 2 1 → M g , 4 . Q 2 u,d ) j Y ≈ Q and c ( X κ R F is the renormalization scale to P m ) i → µ , + Q ) that is realized in a given model. d λ c ( 2 s 2.1 → g LF 2 with the first KK gluon, 2 11 ], the fermion mass hierarchy can be ex- Q µ √ − 15 X , 2 − 2 and g ]. In minimal universal extra dimensions [ 14 ]. In such models, the SM fields are the lowest- ij η is the length of the extra dimension, and δ 8 – 4 – 27 2 for down-type quarks, Λ is an ultraviolet scale 20 13 L / – – L 2 → + 1 16 2 11 1 √ λ = 1 g 1 8 d Y KK L X ]. Since KK parity is absent, the first KK gluon decays to (1) differences in bulk mass parameters. Typically, the KK P M m ) and identifying 2 O structure defined in eq. ( 55 2 , (5–10 TeV) to satisfy low-energy flavor violation probes, espe- √ η 2.1 O 54 ≈ µ Λ ], but this scale can be lowered in the case that the bulk fermions ij 24 , and λ κ log , 2 λ π 1 ]. mixing [ 16 25 2 are the bulk mass parameters for LH and RH quark fields [ 1 K √ = 2 for up-type quarks, d µ − c u γ ¯ Y a K T In Randall-Sundrum warped scenarios [ s g , and u 2.3 Non-universal couplings andAs we flavor have constraints emphasized, massive colorStandard octet Model vectors physics. arise in Their collider numerous and modelson flavor of the physics beyond phenomenology particular the depends crucially Given the stringent constraints on tree-level flavor changing neutral currents [ maximize the top quark wavefunctionwavefunctions overlap for with the the light TeV-scale infrared quarksthe brane first are while KK skewed the towards gluonexceed the preferentially 80% ultraviolet decays [ brane. to top As quarks, a with result, branching fractions that can where RH up-type couplings arecouplings obtained are by obtained replacing byboundary replacing conditions ofc the 5D gluon, reproduce the known SM quark masses, these bulk mass parameters must be chosen to SM zero-mode quarks, andbetween this the coupling is zero given modescoupling by structure and calculating in the the eq. wavefunction ( KK overlap gluon in the extra dimension. Using the general plained by allowing fermions tomass propagate in hierarchy the originates bulk, as wheremass the observed scale charged must fermion thencially be obey a flavor symmetry [ where larger than the inverseevaluate size the of coupling. the extra dimension, and KK particles running in theon loop. These the couplings KK are generatedinvariance gluon from breaking, boundary and and conditions read the bulk masses, which provide the only source of translational Models with extramassive spacetime color dimensions octet vector provide resonances an [ lying states alternative of framework a forfive-dimensional Kaluza-Klein equations realizing tower, of whose motion massesthe [ and level-2 dynamics KK gluon result obtains from a solving coupling the to SM quarks from one-loop diagrams with level-1 2.2 Color octet vectors from extra dimensions JHEP09(2017)101 | , s − D 1 B ˜ 3 λ . C | (2.14) (2.16) (2.18) (2.13) (2.10) (2.11) (2.12) (3 TeV from ≈ − ] 4 60 21 10 – ]. A tree-level TeV and D, 3 × ˜ λ 57 58 , 2 m L 10 . ≈ d 2 † × 51 d , 12 . V 0 > , . u ) D, | 1 )) (2.17) . 50 ) (2.15) V | | , ˜ λ | † , 33 u m R . 33 33 > 33 ˜ λ 24 d † | d ˜ ˜ λ λ ˜ λ † | | d λV , | ], we minimize the impact of | , , u , , | | CKM and Λ | ηU V ) 50 11 ηU d † 11 11 , assuming the other is vanishing: β d 11 u ˜ λ ˜ λV 1 K U | ˜ ˜ λ λ s ˜ λ V U | | 33 | (TeV) scale color octets as long as L C d a ˜ λ = V P , the stronger constraints come from O , giving / , † X . a ˜ CKM µ η requires Λ a m R 22 max( V 11 γ / t max( max( , | X d ˜ mixing [ λ max( 12 2 s β ˜ λ X s d a in the gauge basis. Nevertheless, flavor † ¯ u s s g d = t g s 0 1 2 D, B = g g = , which leads to s M g η † m R ˜ )( λ d g C K ¯ κU d R | 33 α V 1 11 u m L d ˜ s λ 6 u ¯ − ˜ λ d d + U − L V – 5 – 0 U † 6= P m R + u ¯ = , and = µ K u TeV from Re κ γ † m L 22 ˜ 130 GeV 2700 GeV κ u λV 3 1 K 3500 GeV 4000 GeV ), we rotate the quark fields to the mass basis by α ˜ u λ , u ¯ , † d C > > u λ 10 , and V κU † > > u † 2.1 = u u m R X X λV × = ( V X X U u λV u 11 d a M M 1 u 1 V K M M . ˜ λ V = / matrices can be chosen such that the effective interaction V a X 1 O a : : R ≡ / t : : η X = s u a > | | 1 1 K K D g t u s d ˜ λ s ˜ λ C C 1 1 B U B m R g measurements, where u , C C ), using global fit values for the CKM elements [ m L | | , and 0 Re m L Im s ¯ ], u + ¯ are diagonal in the quark mass basis, 11 κ d B ˜ λ η , 57 = , λ − − L ⊃ can be matched to the four-fermion operator [ L 0 s mediates tree-level flavor-changing neutral currents (FCNCs). Since the 56 d [ ¯ 33 µ 240 TeV. Using the tree-level, CKM-induced off-diagonal elements of B d ˜ µ , and ˜ λ † d V X ( κ > X 4 V , , ˜ ], we can constrain the maximum size of u − and m L ˜ λ 1). Moreover, with this structure, V . u 50 10 0 d [ (0 ≡ B = × 1 K L ) − C i u ∼ O 0 3 d CKM u . ¯ ˜ requires Λ we obtain We see that theseλ constraints are easily satisfiedB for Using the requirementIm Λ with the Wilson coefficient and hence strongest FCNC constraints comethese from constraints by assuming 1 exchange of The corresponding LH down quarkV interactions have small, off-diagonal entries induced by We see that the matrices violating effects are stillthe induced quark in mass interactions basis.V of From LH eq. down ( quarks by the rotation to adopt flavor-diagonal couplings for JHEP09(2017)101 ], ! as ij R 25 ]. g (2.21) ij L (2.20) (2.22) (2.19) g 59 CKM , j 2 X m 51 ˜ i , λV m m 2 / 1 † CKM +6 ! V If the masses of ! 2 q 2 2 X 1 , since single pro- = . m m η 2 j 0 2 X 4 ˜ λ m m − . − 1 ) 1). As a result, we can 2 i | 2 X d, u, s, c , which is constrained by . , and ˜ m κ 33 m (0 ˜ λ = ! , ˜ penguin amplitudes, are also | † ˜ . λ R , CKM 1 2 q | g g V s 0 X − , L 11 ∼ O ¯ ˜ λ q g X ˜ λ m q | ˜ ) 2 q λ 2 j 2 X 2 X is 2 R m → m m q m g CKM b , V + 12 ]. We can define max( + 2 / mass, the partial width simplifies to + 6 2 i s 2 X 2 1 L g g m 59 ! m and ! , ( X j 2 s 2 q 2 X γ 4 X 58 m α 1 2 s i 2 m final states are then simply ratios of the corre- – 6 – m m − X m , which we will neglect and hence approximate ¯ t ]. The corresponding bound is 1 t 36 GeV 4 − ) = , while large branching fractions to bottom quarks 33

→ 50 1 − ˜ λ ) > ¯ 33 qq 2 , 2 b

, entirely consistent with flavor bounds. We remark ) κ X ) 11 ij R 33 is diagonal, then the tree-level flavor violating couplings → , and 2 j g ˜ 2 λ R 2 X ˜ b λ M ¯ to a pair of quarks g m b m couplings are aligned in the down-quark sector [ X × + ( , + : X µ 2 − CKM Γ( wavefunction profiles peaked close to the infrared brane [ ) . This is the effective description of the warped extra dimen- 700 TeV [ jj 2 L 1 D 2 i X ij L 2 X g 33 R 11 ˜ g λV ( > C m b η m ˜ λ ((

. −

ji R Im † 1 X CKM g and X ]. (TeV) color octet vectors with dominant branching fractions to either V m = 6 m 12 R s

O s t 59 ij R α α , are the corresponding diagonal entries in or jets, × g 58 R 11 g are at most 5% ) = ) = i and ˜ λ q j ¯ D ji qq L ¯ q g ˜ λ , and j = 1 constraints, including mixing, where Λ → q = i L 0 . The partial width of 33 ¯ q F g ij L ¯ ˜ λ ˜ X λ D g → ≈ Γ( For reference, the generalized flavor violating partial width is − 1 X 0 D Γ( ˜ where sion scenario with and small hierarchies inprecision these tests third [ generation couplings are consistent with electroweak The branching fractions for sponding sum of squaredcan couplings. easily be We realized seecorresponds by that to increasing large increasing ˜ branching ˜ fractions to top quarks where the quarks can be neglected compared to the duction via gluons iscouplings forbidden at tree-level. Inλ our scenario, the induced flavor-violating immediately satisfied if the 2.4 Collider phenomenology ofColor octet color vectors octet can vectors berate singly scales and with doubly produced the at corresponding colliders. partial The width single-production into diagonal, and then theD LH up-quark couples via The ∆ realistically expect tops, that an alternative assumptionparticular, of if the instead flavor structureare can shifted relax to these bounds the further. LH up-quark In couplings [ which are again weakened to the sub-TeV scale for JHEP09(2017)101 ] ] - t ) ) ], b 62 70 jj 68 JJ ( ], in- ¯ t ) and t )( 63 jj ( JJ → ) and 4 ¯ t t ∗ 3 from the . JJ 0 ]. In the case )( algorithm [ XX 38 5 v2.4.3 [ ) T – JJ k b ¯ → 9. We identify R < . b 32 -dependent tagging [ 4 ( η ¯ t pp t t 4 ) signal regions would < | jj → η | )( - and ) final states. ∗ b ¯ T -factor of 1.5, adopted from jj b p MadGraph ) and ( -jets. K ¯ t b XX t jj search and our proposed searches ( ¯ t t t ), and ( -mesons within ∆ ] and ) and B jj 50 GeV and 31 + jets production cross section is known jj – )( ( ¯ t ¯ t b ¯ t > t b 26 T p ), ( and dijet systems. Of course, the main SM ] model using Universal FeynRules Output [ b ¯ – 7 – b ¯ t 61 t )( b ¯ b . Jets are clustered using the anti- b inclusively [ ] for showering and hadronizations. We remark that or b v2.3.26 [ with up to two additional jets at leading order, using j 65 + jets background, where other single boson and diboson ] detector simulation, with a , -factor should not significantly affect our projected results. or ¯ t t = 71 ¯ tj j 64 K t ]. The inclusive SM and its color octet representation. Hence, all searches in J = 67 X , J ). Although there are numerous possibilities for the top decays, b ¯ v8.2 [ m ) mixed decay channels are critical. In particular, the b 66 v3.1.2 [ [ resonance should appear as a resonant peak over a smooth continuum b ( ¯ ¯ t b ), with t ]. Since the signal will rely on tagging two top candidates, we sim- ( FeynRules X ]. We rescale the background by a flat ¯ t decay width is preferred, additional signal discrimination is easily gained t 38 JJ -dependent ), with → 66 b ¯ – ( T b ∗ p Pythia 26 JJ -tags. The orthogonal ( b νjj → 5, and we require jets to have )( decay widths to tops and light quarks are comparable. In the next section, we Delphes . ) and XX X BlackHat X b` ¯ jj JJ v.2.1.0 [ 1%. ( b ( = 0 . + ¯ t → ]. Since our t → → R 69 pp ) mixed decay searches offer substantial improvements in covering the sensitivity gap We construct a As previously highlighted, the single dijet resonance constraints scale with the overal ∗ ∗ b ¯ b ( ¯ t rate is 0 XX with jets using a efficiency of about 70%main jet for axis; displaced the tracks charm from misidentification rate is roughly 15% and the light flavor mistag sion [ background, a 3.1 Event selectionWe strategy first discuss the semi-leptonic top decay channel, where our signal process is ulate the SMSherpa background, Sherpa at next-to-next-to-leading orderwhereas and differential cross next-to-next-to-leading sections can log be obtained (NNLL) at next-to-leading precision order and NNLL [ preci- to perform leading order Monteterfaced Carlo with event simulation with the leading ordersearch calculation limits allows [ a direct comparison to existing ( We analyze pair-produced resonancesand in a new mixedwe decay mainly mode, focus onhandles the for semi-leptonic tagging andbackground fully the is leptonic reconstructible the final irreducible states,+ which jets provide backgrounds clean are subleading after requiring multiple when the describe our collider analyses optimized for the 3 Collider analyses of the mixed channels, where the by requiring then have enhancedsearches. and If complementary the sensitivity coupling toin compared tops the to is preferred, the thent current the 4 ( partial width into lightculable flavor knowing quarks. only pair-production Pair-production rates, modes however, provide are importantonance robustly complementary searches. cal- reach comparedXX to The single current res- LHC analyses focus on the simplest topologies, with JHEP09(2017)101 π jj ≤ 3 → j 1 j X Delphes R 250 GeV, and . To avoid the X . ≥ with ∆ -tagged and one system by adding -tagged jet comes m X b T 3 mode by selecting b b ¯ p j m b 3) b ¯ / b . The upper left panel 3) (4 / 1 (4 ≥ T of the resonant dijet system, | ≥ H ]. T 115 GeV. Again we distinguish . The final signal rates lead to T,j p 80 GeV. Events must also have 72 5, with isolation using 15. This follows the hemisphere mode is optimized by requiring p and add to it the hardest light jet . . 2 | ≤ cut, 2 0 j 1 ≥ j `` jj T < ≤ T m | H p 1 = Σ η mass, which is because of the combina- | T T,j X H /p 2 -jets, lepton, and jets. Difficulties in resolving b . We then reconstruct the distribution coming from the signal jets. The T,j ¯ t p – 8 – t T H 20 GeV and decay, we assume that the leading > b ¯ , when b T T -tagged and untagged jets must have p p b 50 GeV, and keep the -tagged jets, while the decays should be untagged and relatively hard. Adding the b , while the most salient kinematic distributions for the back- . We also add in the next hardest light jet > signal region and vice versa. π signal resonance is extracted from forming the invariant mass 1 jj T bb ≤ / decay modes, we construct the dijet invariant mass as our final E → JJ 2 m j jj 1 j X → R decay directly, not from dijet resonance decay modes, using the same method as the semi-leptonic -tagged, and also require exactly two isolated leptons of opposite charge. X and b targetted modes. Again, the broad peak structure arises mostly from the -tagging efficiency and the combinatorial ambiguity also cause jj b ¯ b ¯ b JJ mode, we start with the leading light jet b b +jets background we veto events with -tagged jets. For the are not balanced in b jj Z → and distribution, however, only offers an overal rate shift from the additional signal shows the hardening of the 2 b ¯ and j X b 1 jj T,JJ 80 GeV, as well as signal mass-optimized p and The search in the fully leptonic top quark decay channel is very similar. We again For both For the For this purpose, we define two signal regions. We target the Naively, the Events must have at least 5 jets, at least two of which must be > 1 which satisfies ∆ j T 2 / two of which are We loosen the MET cut, anticipated between search. The corresponding cut flow is presented in table in the combinatorial ambiguity in capturing theWe correct note signal that jets toevents to reconstruct populate the the resonance. select jets and leptons as in the semi-leptonic channel, but we require only 4 jets, at least ground stacked with different signal hypothesesin are figure shown in figure dijet events and no strong correlationtorial with ambiguity the among signal the jets. The bottom panels show the invariant mass distributions intuition, where the third hardest light jet accounts for the wide-angle final statekinematic radiation of discriminant. our signal The quarks. analysis signal are and shown in background table cut efficiencies for the semileptonic the remaining leading jet,best whether reflects tagged the or dijet untagged. resonance in We spite find of that thej this underlying reconstruction combinatorial ambiguity. if multijet combinatorial ambiguities are discussed in, e.g., [ events with more thanexactly two two from the of the two leadingusing jets. the dijet and The ditop jet massesThus, to the combinatorics, discriminate main the however, goal signal present of fromadvantage a the our of irreducible collider major the background. strategy resonant hurdle is high to against and mass solve the dijet the relevant signal, angular combinatorial spread the ambiguity, between taking large the must be untagged. Thethe leading subleading untagged jet,exactly if one present, isolated lepton must with have default parameters. WeE furthermore cut on missing transverse energy (MET), requiring JHEP09(2017)101 ). ¯ t (3.3) (3.1) (3.2) t → +jets +jets ¯ ¯ t t t t X +jets for the +jets for the ¯ t ¯ t t t searches. We A t = Br( tt ref Background Background , 5.8 5.8 5.8 1.23 0.71 0.39 0.75 0.75 0.75 21% 11% 2.7% 37% 37 % 37% 32% 19% 10% 64% 64% 64% 91% 91% 91% 2 qq, 0.053 0.027 0.007 ) 1.3 TeV 1.5 TeV 1.7 TeV 1.3 TeV 1.5 TeV 1.7 TeV ) and 4 Γ tot, width Γ JJ ) = 50%. ) = 50%. ) searches in combination JJ ) projected exclusion after 2 JJ )( JJ JJ (Br JJ ( . Br JJ ¯ t × → → ) ( JJ t ¯ t t X ref X X JJ σ m | ) = → ∗ and dominant background Signal Signal and dominant background A X ) = Br( ) = Br( X ¯ ¯ t t XX X JJ t t m Br( m ), respectively, where Br Br → → → tt − 1.06 0.31 0.09 1.52 0.45 0.13 63% 57% 48% 66% 68% 70% 83% 79% 76% 84% 87% 89% 96% 96% 97% 0.059 0.017 0.003 0.148 0.045 0.009 X X 1.3 TeV 1.5 TeV 1.7 TeV 1.3 TeV 1.5 TeV 1.7 TeV pp Br – 9 – ( width σ JJ σ ) = 1 2; ¯ t only decays to quark pairs, we can express the pair = t constraint and the = ≥ X t b X 20 GeV) 20 GeV) X → N m | m > > ) | 1, 2; X ) and 2(Br T,` T,` ≥ ≥ JJ p p res j b 2 ) Br( ) )( N N tt ). The 4 JJ JJ ( ( JJ 5 with 4 with 250 GeV; 250 GeV; → excl → ≥ ≥ > > σ pp J J with (Br ( 5% additional contribution compared to the semi-leptonic channel. X N N 2 ) ≈ leading T,b leading T,b excl σ JJ , p , p X X X X = Br( m m m m 3) 3) leading T,j leading T,j JJ . Cut flow for different resonance masses . Cut flow for a different resonance masses / / p p 115 GeV (4 (4 80 GeV 50 GeV ≥ The single dijet resonance limits are determined only after specifying the total width ≥ ≥ > > = 1; = 2; `` T T ` ` T T / / Remaining cross section [fb] H Remaining cross section [fb] H m E E N N Event selection [fb] ( Event selection [fb] ( Signal mass Signal mass Fully Leptonic Search Semi-Leptonic Search of the resonance. Ifthe the partial total width width into is light narrow, quarks. a We reference see cross that section can be rescaled by So, the pair production limits can be translated according to: with Br replacing (Br also show the singleassume production that our limits new forproduction physics dijet constraints state in and the ditop branching resonance fraction vs. searches. mass plane, Since where we the same relative signal to backgroundrate ratios is as the only semi-leptonic an analysis, but the absolute 3.2 Comparison withWe current now searches compare the projectedwith sensitivity the from recasted the mixed exclusions from ATLAS and CMS for ( Table 2 fully leptonic search. All branchingsections. ratios We are normalize applied the to signal signal assuming and Br( background when quoting cross Table 1 semi-leptonic search. All branching ratiossections. are We applied normalize to the signal signal and assuming background when Br( quoting cross JHEP09(2017)101 (3.4) (upper [GeV] [GeV] bb )=50% )=50% T,JJ t t m p t t T,JJ → → p . =1.3 TeV =1.5 TeV =1.7 TeV =1.3 TeV =1.5 TeV =1.7 TeV X X X X X X JJ)=BR(X JJ)=BR(X ref → → B+S m B+S m B+S m B+S m B+S m B+S m Background only (B) Background only (B) Background only qq, Γ BR(X BR(X tot, width Γ 5 TeV signal (blue, solid), (upper left), . tt T = 1 H ) Br X tt m Br − (1 + jets background (red, dashed), stacked ref ¯ t t σ 0 200 400 600 800 1000 1200 1400 1600 1800 2000 0 500 1000 1500 2000 2500 3000 0 0 .

0.1 0.1

T,JJ 0.5 0.4 0.3 0.2 0.8 0.7 0.6 0.5 0.4 0.3 0.2 bb

[fb/(100 GeV)] [fb/(100 dm / d [fb/(67 GeV)] [fb/(67 dp / d σ 2 σ tt Br – 10 – resonance constraint follows ¯ t t [GeV] [GeV] jj to show the unsculpted dijet invariant mass spectra. T width m H )=50% )=50% t t σ t t T → → H ≥ =1.3 TeV =1.5 TeV =1.7 TeV =1.3 TeV =1.5 TeV =1.7 TeV X X X X X X X (lower right), where the invariant mass definitions are described m | JJ)=BR(X JJ)=BR(X ) bb → → B+S m B+S m B+S m B+S m B+S m B+S m Background only (B) Background only (B) Background only m res ) BR(X BR(X ¯ t t ( 7 TeV signal (black, solid). Differential distributions are presented after jet cut 3 TeV signal (green, solid), background + . T . H → = 1 = 1 pp resonances, the above constraint becomes a bounded requirement on the cuts but before the ( X ¯ t X t T m m excl / E σ (lower left), and . Differential distributions in the semi-leptonic analysis for jj m 0 500 1000 1500 2000 2500 3000 0 0 500 1000 1500 2000 2500 3000 3500 4000 4500 5000

invariant mass shapes, where we assume a 10% systematic uncertainty on signal and

0.1 0.1

0.7 0.6 0.5 0.4 0.3 0.2 0.8 0.7 0.6 0.5 0.4 0.3 0.2

T jj

/ dH / d [fb/(150 GeV)] [fb/(150 / dm / d [fb/(100 GeV)] [fb/(100 σ σ Note that here we dropwhen the presenting acceptance their factor results. sinceleptonic the We and experiments combine fully unfold all leptonic the search fourJJ acceptance and orthogonal compute signal the regions 95% C.L. ofbackground. limits the based The semi- on result the can respective be found in ﬁgure In the case of branching fraction to tops. Hence, the right), in the main text.background + We show distributionsbackground + for the SM selection and Figure 1 JHEP09(2017)101 −

BR(X→ t )t ]. ) = 1 59 , 1 0 JJ 0.1 0.2 0.3 0.4 0.5 0.6 0.7 0.8 0.9 58 , → 51 -1 X ] are absent from -4 [GeV] X 47 ]. The corresponding m , corresponds to diag- of integrated luminosity, . Any direct resonance =5x10 1 X 48 X X − m (JJ), 3000 fb /m 4 t X t /m − Γ X , such LH quark couplings to 10 . We also show current limits from 1 × 2.3 − -1 , and 300 fb ] searches. 1 = 5 − resonance limits [ 40 , X ¯ JJ (ATLAS), t 300 fb t 39 allows complementary dijet constraints from , 100 fb 1 4 − − -1 – 11 – JJ (CMS) 10 ) (green) [ × 100 fb JJ 1 TeV. On the other hand, these couplings generally -1 = 5 > X 37 fb X ], and ( (JJ)(JJ) m /m 31 X 4t 1. As discussed in subsection . ]. We remark that the 0 . 40 , η ) (blue) [ 39 , ˜ κ searches could in principle be evaded completely with a suitably small JJ 1200 1400 1600 1800 2000 2200 , ˜ )( ˜ λ JJ JJ , but choosing Γ X ], ( ). We show our limit in black for 37 fb ¯ . Exclusion limits for diﬀerent resonance masses as a function of Br( t 1 38 t 0

0.1

0.9 0.8 0.7 0.6 0.5 0.4 0.3 0.2 BR(X JJ) → → As mentioned previously, the sensitivity from single production compared to the sen- We remark that the width of our resonance, Γ X readily satisfy flavor violation bounds from meson oscillation measurements and neu- (red) [ t CMS and ATLAS [ model-dependent, but realistic and complete scenarios can be constructedsitivity from [ pair production stronglybounds depends from on the ratiochoice Γ of Γ onal entries of X tral current transitions given arise from mixing thetivity SM in quarks the with parentflavor heavy violation extended vectorlike bounds, color states, collider constraints, gauge since electroweak precision symmetry otherwise observable tests is perturba- are violated more [ Br( as well as the expected4 sensitivity at the HL-LHC with 3000 fb Figure 2 JHEP09(2017)101 ] 4 bb − 38 [ 10 t ) and × jj 7 ) search ) = Br ( b ¯ t ¯ t b & JJ ] and 4 X )( → 31 ) search would b ¯ /m X JJ b )[ X to reach a similar )( corners. The mass t b ¯ JJ b tt )( decay channels for pair ) mass window to test ) channels. b ¯ JJ as a function of the three b jj jj ) and 4 decay channels are compared. X )( and Br b ¯ m JJ jj b . 1 )( JJ , and − b ¯ b JJ , and , b ¯ ¯ t b ) and ( resonance limit is symmetric around t b ¯ , ¯ t ¯ t b t t )( b ¯ ) search to explore. Our search will probe b indicates which particular dedicated search are therefore from ( JJ 3 ), the ( 2 ¯ t corners at 3 ab t – 12 – 3.4 tt -tagged backgrounds would be required to suitably b , allowing both branching fractions Br( ) signal regions. In particular, the ( 3 and Br jj JJ )( . These constraints are only relevant once Γ 4 jj − 10 × ), and ( = 5 jj searches. X )( shows the lower limit on the resonance mass t b ¯ b , we assume that all quark couplings are flavour universal except for the top. /m 3 branching fractions must equal 100% in our model. The shading in the left ], where the main novelty would be varying the ( 2 X ¯ t ), ( t b ¯ 74 , b to float. The results are presented in an equilateral triangle since the sum of the . Left: strongest mass limits when the various ) and 4 around 1 TeV. As shown in eq. ( )( for Γ 73 tt b and ¯ JJ 2 X b b ¯ = 50% since the maximum rate in this channel corresponds to equal partial widths to ), overtake the sensitivity in the central areas of the triangle compared to the existing We reiterate that a complete characterization of In figure The strongest existing bounds in figure )( b m b ¯ b tt , ( JJ ¯ t Higgs [ for new resonances.and The thus substantial multijet statistics background,smooth in however, paired the is invariant mass very spectrum challenging in to the ( simulate t ( production colored resonances wouldinto necessitate ( optimizing thebear current ( striking similarities with the current searches for pair production of the 125 GeV and Br jj panel of figure branching fractions. The right panelyields of the figure corresponding lower mass limit. We see that our new search channels, leaving significant room for ourmasses dedicated of up to 2sensitivity TeV in at the the respective HL-LHC. Br We expect the ( We relax this assumption in figure Br dijets and ditops. searches, which are clearlyreach optimal of for both their respective searches Br weakens by about 250 GeV in the intermediate regime, however, Figure 3 Right: search region that gives the best sensitivity. figure for JHEP09(2017)101 , , plane, X m ) resonance ¯ t t vs. JJ ]. SPIRE mass is above 1 TeV and its IN ) searches will fill a sensitivity X ][ b ¯ b ( ]. ¯ t t ) mixed decay channels of a mas- b ¯ b ( ¯ t SPIRE t New strong interactions at the Tevatron? ) and IN ][ jj ( ¯ t t ) and arXiv:1010.4309 jj – 13 – [ ( ]. ¯ t t searches. This gap is clear in the Br 1. As a result, the LHC provides the leading reach to SPIRE . t IN hep-ph/9603311 ), which permits any use, distribution and reproduction in [ (2010) 085 resonance to light quarks, bottom pairs, or top pairs are Colored Resonant Signals at the LHC: Largest Rate and [ X 12 ) and 4 JJ JHEP (1991) 419 (1996) 92 )( CC-BY 4.0 , JJ This article is distributed under the terms of the Creative Commons ) analyses, we focused on resolving the jet combinatorial ambiguity to B 266 B 380 JJ Topcolor: Top quark condensation in a gauge extension of the standard model ( ¯ t t Simplest Topology Phys. Lett. Phys. Lett. Nevertheless, our results show that new In our C.T. Hill, R.S. Chivukula, A.G. Cohen and E.H. Simmons, T. Han, I. Lewis and Z. Liu, [2] [3] [1] Attribution License ( any medium, provided the original author(s) and source areReferences credited. is supported by the ClusterStructure of of Excellence Matter Precision (PRISMA-EXC Physics, 1098). FundamentalGerman Interactions The Research and Foundation work (DFG) of in MB theat is framework the moreover of supported Large the by Hadron Research the Unit Collider” “New (FOR Physics 2239). Open Access. FY would like to thank R.during Sekhar Chivukula the and Elizabeth 2015 Simmons LesInstitute for helpful Houches for discussions summer Theoretical Physics, session,scientific “The and program. TeV also FY Scale: would Susanneat also A Westhoff Fermi like Threshold at National to to the Accelerator acknowledge New the Laboratory Mainz Physics?” hospitality while of this 2017 the work theory was group completed. This research resonance greatly benefitsproduction from modes this combined with complementary different decayunderlying information, channels Lagrangian provide where direct couplings. information single about and pair Acknowledgments signal discrimination in this regard. gap between the ( which itself provides asearches useful of tool pair-produced for resonances. easily presenting We the stress results that from a different post-discovery collider scenario of a new TeV-scale color octet vectorsvirtue with of variable the couplings model to independent heavy pair and production light rate. flavorreconstruct quarks the by dijet or dibottomis resonance. also In possible, principle, but reconstructing the our ( scenario with its many resolved jets did not afford any additional In this work, wesive, have color highlighted octet the vectorunderlying as couplings new of targets the forentirely consistent ATLAS with and low CMS energycouplings searches. FCNC constraints to Hierarchies if quarks the in are the at most 0 4 Conclusion JHEP09(2017)101 , ]. ]. ]. B , Phys. JHEP , , , (2007) SPIRE SPIRE (1999) Phys. SPIRE IN , IN ¯ IN t 09 t ][ 83 Phys. Rev. ][ ][ , (2001) 095010 → Phys. Lett. ¯ p , (1985) 430 p JHEP ]. , D 64 ]. Topcolor in the LHC ]. B 153 SPIRE SPIRE SPIRE IN ]. Phys. Rev. Lett. IN IN ][ Bulk standard model in the hep-ph/9912498 arXiv:0906.4525 , arXiv:0911.2955 ][ ][ [ [ Phys. Rev. [ , ]. SPIRE ]. IN ]. Phys. Lett. , ][ ]. SPIRE IN SPIRE (2010) 294 SPIRE (2009) 1897 IN ][ Bounds on universal extra dimensions IN (2000) 084025 ][ SPIRE hep-ph/0012259 ][ IN [ hep-ph/0006041 hep-ph/0201300 Collider implications of universal extra Experimental probes of localized gravity: On and Bulk gauge fields in the Randall-Sundrum model [ A 24 [ ][ B 683 ]. ]. 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