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The European Physical Journal. C, Particles and Fields
 
Eur Phys J C Part Fields. 2017; 77(7): 450.
Published online 2017 July 6. doi:  10.1140/epjc/s10052-017-4962-y
PMCID: PMC5512613

Excited scalar and pseudoscalar mesons in the extended linear sigma model

Abstract

We present an in-depth study of masses and decays of excited scalar and pseudoscalar q¯q states in the Extended Linear Sigma Model (eLSM). The model also contains ground-state scalar, pseudoscalar, vector and axial-vector mesons. The main objective is to study the consequences of the hypothesis that the f0(1790) resonance, observed a decade ago by the BES Collaboration and recently by LHCb, represents an excited scalar quarkonium. In addition we also analyse the possibility that the new a0(1950) resonance, observed recently by BABAR, may also be an excited scalar state. Both hypotheses receive justification in our approach although there appears to be some tension between the simultaneous interpretation of f0(1790)/a0(1950) and pseudoscalar mesons η(1295), π(1300), η(1440) and K(1460) as excited q¯q states.

Introduction

One of the most important features of strong interaction is the existence of the hadron spectrum. It emerges from confinement of quarks and gluons – degrees of freedom of the underlying theory, Quantum Chromodynamics (QCD) – in regions of sufficiently low energy where the QCD coupling is known to be large [14]. Although the exact mechanism of hadron formation in non-perturbartive QCD is not yet fully understood, an experimental fact is a very abundant spectrum of states possessing various quantum numbers, such as for example isospin I, total spin J, parity P and charge conjugation C.

This is in particular the case for the spectrum of mesons (hadrons with integer spin) that can be found in the listings of PDG – the Particle Data Group [5]. In the scalar channel (JP = 0+), the following states are listed in the energy region up to approximately 2 GeV:

f0(500)/σ,K0(800)/κ,a0(980),f0(980),f0(1370),K0(1430),a0(1450),f0(1500),f0(1710),K0(1950),a0(1950),f0(2020),f0(2100).

The pseudoscalar channel (JP = 0-) is similarly well populated:

π,K,η,η(958),η(1295),π(1300),η(1405),K(1460),η(1475),η(1760),π(1800),K(1830).

A natural expectation founded in the Quark Model (see Refs. [6, 7]; for a modern and modified version see for example Refs. [8, 9]) is that the mentioned states can effectively be described in terms of constituent quarks and antiquarks – ground-state q¯q resonances. In this context, we define ground states as those with the lowest mass for a given set of quantum numbers I, J, P and C. Such a description is particularly successful for the lightest pseudoscalar states π, K and η.

However, this cannot be the full picture as the spectra contain more states than could be described in terms of the ground-state q¯q structure. A further natural expectation is then that the spectra may additionally contain first (radial) excitations of q¯q states, i.e., those with the same quantum numbers but with higher masses. (In the spectroscopic notation, the excited scalar and pseudoscalar states correspond, respectively, to the 2 3P0 and 2 1S0 configurations.) Of course, the possibility to study such states depends crucially on the identification of the ground states themselves; in the case of the scalar mesons, this is not as clear as for the pseudoscalars. Various hypotheses have been suggested for the scalar-meson structure, including meson–meson molecules, q¯q¯qq states and glueballs, bound states of gluons – see, e.g., Refs. [1076]. Results of these studies are at times conflicting but the general conclusion is nonetheless that the scalar q¯q ground states (as well as the glueball and the low-energy four-quark states) are well defined and positioned in the spectrum of particles up to and including the f0(1710) resonance.

The main objective of this work is then to ascertain which properties the excited scalar and pseudoscalar q¯q states possess and whether they can be identified in the physical spectrum.

Our study of the excited mesons is based on the Linear Sigma Model [7780]. This is an effective approach to low-energy QCD – its degrees of freedom are not quarks and gluons of the underlying theory but rather meson fields with various values of I, J, P and C.

There are several advantages that the model has to offer. Firstly, it implements the symmetries of QCD as well as their breaking (see Sect. 2 for details). Secondly, it contains degrees of freedom with quantum numbers equal to those observed experimentally and in theoretical first-principles spectra (such as those of lattice QCD). This combination of symmetry-governed dynamics and states with correct quantum numbers justifies in our view the expectation that important aspects of the strong interaction are captured by the proposed model. Note that the model employed in this article is wide-ranging in that it contains the ground-state scalar, pseudoscalar, vector and axial-vector q¯q states in three flavours (u, d, s), the scalar dilaton (glueball) and the first excitations in the three-flavour scalar and pseudoscalar channels. Considering isospin multiplets as single degrees of freedom, there are 16 q¯q ground states and 8 q¯q excited states plus the scalar glueball in the model. For this reason, it can be denoted the “Extended Linear Sigma Model” (eLSM). A further advantage of eLSM is that the inclusion of degrees of freedom with a certain structure (such as q¯q states here) allows us to test the compatibility of experimentally known resonances with such structure. This is of immediate relevance for experimental hadron searches such as those planned at PANDA@FAIR [81].

With regard to vacuum states, the model has been used in studies of two-flavour q¯q mesons [82], glueballs [8387], K1 and other spin-1 mesons [88, 89] and baryons [90]. It is, however, also suitable for studies of the QCD phase diagram [9193]. In this article, we will build upon the results obtained in Refs. [94, 95] where ground-state q¯q resonances and the glueball were considered in vacuum. Comparing experimental masses and decay widths with the theoretical predictions for excited states, we will draw conclusions on structure of the observed states; we will also predict more than 35 decays for various scalar and pseudoscalar resonances (see Sect. 3.3).

Irrespective of the above advantages, we must note that the model used in this article also has drawbacks. There are two that appear to be of particular importance.

Firstly, some of the states that might be of relevance in the region of interest are absent. The most important example is the scalar glueball whose mass is comparable [54, 58, 61, 64, 65] to that of the excited q¯q states discussed here. The implementation of the scalar glueball is actually straightforward in our approach (see Sect. 2) but the amount of its mixing with excited states is as yet unestablished, mainly due to the unfortunate lack of experimental data (discussed in Sect. 2.3.1).

Secondly, our calculations of decay widths are performed at tree level. Consequently, unitarity corrections are not included. A systematic way to implement them is to consider mesonic loops and determine their influence on the pole positions of resonances. Substantial shift of the pole position may then improve (or spoil) the comparison to the experimental data. However, the results of Ref. [96] suggest that unitarity corrections are small for resonances whose ratio of decay width to mass is small as well. Since such resonances are present in this article (see Sect. 3.3.3), the corrections will not be considered here.

Excited mesons were a subject of interest already several decades ago [97, 98]; to date, they have been considered in a wide range of approaches including QCD models/chiral Lagrangians [99104], Lattice QCD [105110], Bethe-Salpeter equation [111114], NJL Model and its extensions [115125], light-cone models [126], QCD string approaches [127] and QCD domain walls [128]. Chiral symmetry has also been suggested to become effectively restored in excited mesons [129, 130] rendering their understanding even more important. A study analogous to ours (including both scalar and pseudoscalar excitations and their various decay channels) was performed in extensions of the NJL model [117119, 121, 122]. The conclusion was that f0(1370), f0(1710) and a0(1450) are the first radial excitations of f0(500), f0(980) and a0(980). However, this is at the expense of having very large decay widths for f0(1370), f0(1500) and f0(1710); in our case the decay widths for f0 states above 1 GeV correspond to experimental data but the resonances are identified as quarkonium ground states [94].

The outline of the article is as follows. The general structure and results obtained so far regarding ground-state q¯q resonances are briefly reviewed in Sects. 2.1 and 2.2. Building upon that basis, we present the Lagrangian for the excited states and discuss the relevant experimental data in Sect. 2.3. Two hypotheses are tested in Sect. 3: whether the f0(1790) and a0(1950) resonances can represent excited q¯q states; the first one is not (yet) listed by the PDG but has been observed by the BES II and LHCb Collaborations [131, 132] and is discussed in Sect. 2.3.1. We also discuss to what extent it is possible to interpret the pseudoscalar mesons η(1295), π(1300), η(1440) and K(1460) as excited states. Conclusions are presented in Sect. 4 and all interaction Lagrangians used in the model can be found in Appendix A. Our units are ħc = 1; the metric tensor is gμν diag( + ,  - ,  - ,  - ).

The model

General remarks

A viable effective approach to phenomena of non-perturbative strong interaction must implement the symmetries present in the underlying theory, QCD. The theory itself is rich in symmetries: colour symmetry SU(3)c (local); chiral U(Nf)L × U(Nf)R symmetry (L and R denote the ’left’ and ’right’ components and Nf the number of quark flavours; global, broken in vacuum spontaneously by the non-vanishing chiral condensate q¯q [133, 134], at the quantum level via the axial U(1)A anomaly [135] and explicitly by the non-vanishing quark masses); dilatation symmetry (broken at the quantum level [136, 137] but valid classically in QCD without quarks); CPT symmetry (discrete; valid individually for charge conjugation C, parity transformation P and time reversal T); Z3 symmetry (discrete; pertaining to the centre elements of a special unitary matrix of dimension Nf × Nf; non-trivial only at non-zero temperatures [138143]) – all of course in addition to the Poincaré symmetry.Terms entering the Lagrangian of an effective approach to QCD should as a matter of principle be compatible with all symmetries listed above. Our subject is QCD in vacuum. In this context, we note that the colour symmetry is automatically fulfilled since we will be working with colour-neutral degrees of freedom; the structure and number of terms entering the Lagrangian are then restricted by the chiral, CPT and dilatation symmetries.

The eLSM Lagrangian has the following general structure:

ℒ = ℒdil. + ℒ0 + ℒE
1

and in Sects. 2.2 and 2.3 we discuss the structure of the Lagrangians contributing to as well as their matter content.

Ground-state Quarkonia and Dilaton: Lagrangian and the matter content

This section contains a brief overview of the results obtained so far in the Extended Linear Sigma Model that contains Nf = 3 scalar, pseudoscalar, vector and axial-vector quarkonia and the scalar glueball. The discussion is included for convenience of the reader and in order to set the basis for the incorporation of the excited quarkonia (Sect. 2.3). All details can be found in Refs. [94, 95].

In Eq. (1), dil implements, at the composite level, the dilatation symmetry of QCD and its breaking [144149]:

Ldil.=12(μG)2-14mG2Λ2G4lnG2Λ2-G44
2

where G represents the dilaton field and Λ is the scale that explicitly breaks the dilatation symmetry. Considering fluctuations around the potential minimum G0 ≡ Λ leads to the emergence of a particle with JPC = 0++ – the scalar glueball [83, 95].

Terms that (i) are compatible in their structure with the chiral, dilatation and CPT symmetries of QCD and (ii) contain ground-state scalar, pseudoscalar, vector and axial-vector quarkonia with Nf = 3 and the dilaton are collected in the 0 contribution to Eq. (1), as in Refs. [82, 94, 95]:

L0=Tr[(DμΦ)(DμΦ)]-m02GG02Tr(ΦΦ)-λ1[Tr(ΦΦ)]2-λ2Tr(ΦΦ)2-14Tr(Lμν2+Rμν2)+TrGG02m122+Δ×(Lμ2+Rμ2)+Tr[H(Φ+Φ)]+Tr(ΦΦE0+ΦΦE0)+c1(detΦ-detΦ)2+ig22(Tr{Lμν[Lμ,Lν]}+Tr{Rμν[Rμ,Rν]})+h12Tr(ΦΦ)Tr(Lμ2+Rμ2)+h2Tr[|LμΦ|2+|ΦRμ|2]+2h3Tr(LμΦRμΦ)+g3[Tr(LμLνLμLν)+Tr(RμRνRμRν)]+g4[TrLμLμLνLν+TrRμRμRνRν]+g5TrLμLμTrRνRν+g6[Tr(LμLμ)Tr(LνLν)+Tr(RμRμ)Tr(RνRν)].
3

In Eq. (3), the matrices Φ, Lμ, and Rμ represent the scalar and vector nonets:

Φ=i=08(Si+iPi)Ti=12×(σN+a00)+i(ηN+π0)2a0++iπ+K0++iK+a0-+iπ-(σN-a00)+i(ηN-π0)2K00+iK0K0-+iK-K¯00+iK¯0σS+iηS,
4

Lμ=i=08(Viμ+Aiμ)Ti=12×ωN+ρ02+f1N+a102ρ++a1+K++K1+ρ-+a1-ωN-ρ02+f1N-a102K0+K10K-+K1-K¯0+K¯10ωS+f1Sμ,
5

Rμ=i=08(Viμ-Aiμ)Ti=12×ωN+ρ02-f1N+a102ρ+-a1+K+-K1+ρ--a1-ωN-ρ02-f1N-a102K0-K10K--K1-K¯0-K¯10ωS-f1Sμ,
6

where Ti (i = 0, …, 8) denote the generators of U(3), while Si represents the scalar, Pi the pseudoscalar, Viμ the vector, Aiμ the axial-vector meson fields. (Note that we are using the non-strange–strange basis defined as φN=132φ0+φ8 and φS=13φ0-2φ8 with φ(Si,Pi,Viμ,Aiμ).)

Furthermore,

DμΦ ≡ μΦ - ig1(LμΦ - ΦRμ)
7

is the derivative of Φ transforming covariantly with regard to the U(3)L × U(3)R symmetry group; the left-handed and right-handed field strength tensors Lμν and Rμν are, respectively, defined as

LμνμLν-νLμ,
8

RμνμRν-νRμ.
9

The following symmetry-breaking mechanism is implemented:

  • The spontaneous breaking of the U(3) × U(3) chiral symmetry requires setting m02<0.
  • The explicit breaking of the U(3) × U(3) chiral as well as dilatation symmetries is implemented by terms describing non-vanishing quark masses: H diag{hNhNhS}, Δ =  diag{0, 0, δS} and E0 diag{0, 0, ϵS}.
  • The U(1)A (chiral) anomaly is implemented by the determinant term c1(detΦ-detΦ)2 [150, 151].

We also note the following important points:

  • All states present in the Lagrangian (3), except for the dilaton, possess the q¯q structure [82, 152]. The argument is essentially based on the large-Nc behaviour of the model parameters and on the model construction in terms of the underlying (constituent) quark fields. The ground-state Lagrangian (3) contains a pseudoscalar field assigned to the pion since it emerges from spontaneous breaking of the (chiral) U(3) × U(3) symmetry. Furthermore, the vector meson decaying into 2π is identified with the rho since the latter is experimentally known to decay into pions with a branching ratio of slightly less than 1. Pion and rho can be safely assumed to represent (very predominant) q¯q states and hence the large-Nc behaviour of their mass terms has to be Nc0. Additionally, the rho-pion vertex has to scale as Nc-1/2 since the states are quarkonia. Then, as shown in Ref. [82], this is sufficient to determine the large-Nc behaviour of all ground-state model parameters and of the non-strange and strange quark condensates. As a consequence, the masses of all other ground states scale as Nc0 and their decay widths scale as 1/Nc. For this reason, we identify these degrees of freedom with q¯q states. A further reason is that all states entering the matrix Φ in Eq. (4) can be decomposed in terms of (constituent) quark currents whose behaviour under chiral transformation is such that all terms in the Lagrangian (except for symmetry-breaking or anomalous ones) are chirally symmetric [152]. Note that our excited-state Lagrangian (16) will have exactly the same structure as the ground-state one. Considering the above discussion, we conclude that its degrees of freedom also have the q¯q structure.
  • The number of terms entering Eq. (3) is finite under the requirements that (i) all terms are dilatationally invariant and hence have mass dimension equal to four, except possibly for those that are explicitly symmetry breaking or anomalous, and (ii) no term leads to singularities in the potential in the limit G → 0 [153].
  • Notwithstanding the above point, the glueball will not be a subject of this work – hence G ≡ G0 is set throughout this article. With regard to the ground-state mesons, we will be relying on Ref. [94] since it contains the latest results from the model without the glueball. (For the model version with three-flavour q¯q states as well as the scalar glueball; see Ref. [95].)
  • There are two scalar isospin-0 fields in the Lagrangian (3): σNn¯n (n: u and d quarks, assumed to be degenerate) and σSs¯s. Spontaneous breaking of the chiral symmetry implies the existence of their respective vacuum expectation values ϕN and ϕS. As described in Ref. [94], shifting of σN,S by ϕN,S leads to the mixing of spin-1 and spin-0 fields. These mixing terms are removed by suitable shifts of the spin-1 fields that have the following general structure:
    Vμ → VμZSwVμS
    10
    where Vμ and S, respectively, denote the spin-1 and spin-0 fields. The new constants ZS and wV are field-dependent and read [94]
    wf1N=wa1=g1ϕNma12wf1S=2g1ϕSmf1S2wK=ig1(ϕN-2ϕS)2mK2wK1=g1(ϕN+2ϕS)2mK12,
    11
    Zπ=ZηN=ma1ma12-g12ϕN2ZK=2mK14mK12-g12(ϕN+2ϕS)2,
    12
    ZηS=mf1Smf1S2-2g12ϕS2ZK0=2mK4mK2-g12(ϕN-2ϕS)2.
    13
    As demonstrated in Ref. [94], ϕN and ϕS are functions of Zπ and ZK as follows:
    ϕN=Zπfπ
    14
    ϕS=2ZKfK-ϕN/2
    15
    where fπ and fK, respectively, denote the pion and kaon decay constants.

The ground-state mass terms can be obtained from Lagrangian (3); their explicit form can be found in Ref. [94] where a comprehensive fit of the experimentally known meson masses was performed. Fit results that will be used in this article are collected in Table Table1.1. The following is of importance here:

  • Table Table11 contains no statement on masses and assignment of the isoscalar states σN and σS. The reason is that their identification in the meson spectrum is unclear due to both theoretical and experimental uncertainties [154, 155]. In Ref. [94], the preferred assignment of σN was to f0(1370), not least due to the best-fit result mσN = 1363 MeV. The resonance σS was assigned to f0(1710). Note that a subsequent analysis in Ref. [95], which included the scalar glueball, found the assignment of σS to f0(1500) more preferable; f0(1710) was found to be compatible with the glueball. These issues will be of secondary importance here since no mixing between excited and ground states will be considered. (We also note that decays of the excited states into f0(1500) and f0(1710) would be kinematically forbidden. Excited-state masses are discussed in Sect. 3).
  • Table Table11 also contains no statement on the axial-vector kaon K1. Reference [94] obtained mK1 = 1282 MeV as the best-fit result. One needs to note, however, that PDG listings [5] contain two states to which our K1 resonance could be assigned: K1(1270) and K1(1400). Both have a significant mutual overlap [156159, 161, 161174]; analysis from the Linear Sigma Model suggests that our K1 state has a larger overlap with K1(1400) [89]. Nonetheless, we will use mK1 = 1282 MeV for decays of excited states involving K1 – this makes no significant difference to our results since the decays with K1 final states are phase-space suppressed for the mass range of excited mesons.
  • The states η and η arise from mixing of ηN and ηS in Lagrangian (3). The mixing angle is θη =  - 44.6 [94]; see also Refs. [175183].

Table 1
Best-fit results for masses of ground-state mesons and pseudoscalar decay constants present in Eq. (3), obtained in Ref. [94]. The values in the third column will be used in this article in order for us to remain model-consistent. Note that the errors ...

Excited scalars and pseudoscalars

Lagrangian

With the foundations laid in the previous section, the most general Lagrangian for the excited scalar and pseudoscalar quarkonia with terms up to order four in the naive scaling can be constructed as follows:

LE=Tr[(DμΦE)(DμΦE)]+αTr[(DμΦE)(DμΦ)+(DμΦ)(DμΦE)]-(m0)2GG02Tr(ΦEΦE)-λ0GG02Tr(ΦEΦ+ΦΦE)-λ1Tr(ΦEΦE)Tr(ΦΦ)-λ2Tr(ΦEΦEΦΦ+ΦEΦEΦΦ)-κ1Tr(ΦEΦ+ΦΦE)Tr(ΦΦ)-κ2[Tr(ΦEΦ+ΦΦE)]2-κ3Tr(ΦEΦ+ΦΦE)Tr(ΦEΦE)-κ4[Tr(ΦEΦE)]2-ξ1Tr(ΦEΦΦΦ+ΦEΦΦΦ)-ξ2Tr(ΦEΦΦEΦ+ΦΦEΦΦE)-ξ3Tr(ΦΦEΦEΦE+ΦΦEΦEΦE)-ξ4Tr(ΦEΦE)2+Tr(ΦEΦEE1+ΦEΦEE1)+c1[(detΦ-detΦE)2+(detΦ-detΦE)2]+c1E(detΦE-detΦE)2+h12Tr(ΦEΦ+ΦΦE)Tr(Lμ2+Rμ2)+h1E2Tr(ΦEΦE)Tr(Lμ2+Rμ2)+h2Tr(ΦELμLμΦ+ΦLμLμΦE+RμΦEΦRμ+RμΦΦERμ)+h2ETr[|LμΦE|2+|ΦERμ|2]+2h3Tr(LμΦERμΦ+LμΦRμΦE)+2h3ETr(LμΦERμΦE).
16

The particle content of the Lagrangian is the same as the one in Eqs. (5) and (6) for spin-1 states and it is analogous to Eq. (4) for (pseudo)scalars:

ΦE=12×(σNE+a00E)+i(ηNE+π0E)2a0+E+iπ+EK0+E+iK+Ea0-E+iπ-E(σNE-a00E)+i(ηNE-π0E)2K00E+iK0EK0-E+iK-EK¯00E+iK¯0EσSE+iηSE.
17

The covariant derivative DμΦE is defined analogously to Eq. (7):

DμΦEμΦE-ig1E(LμΦE-ΦERμ)
18

and we also set E1 diag{0,0,ϵSE}.

Spontaneous symmetry breaking in the Lagrangian for the excited (pseudo)scalars will be implemented only by means of condensation of ground-state quarkonia σN and σS, i.e., as a first approximation, we assume that their excited counterparts σNE and σSE do not condense.1 As a consequence, there is no need to shift spin-1 fields or renormalise the excited pseudoscalars as described in Eqs. (10)–(11).

We now turn to the assignment of the excited states. Considering isospin multiplets as single degrees of freedom, there are 8 states in Eq. (17): σNE, σSE, a0E and K0E (scalar) and ηNE, ηSE, πE and KE (pseudoscalar); the experimental information on states with these quantum numbers is at times limited or their identification is unclear:

  • Seven states are listed by the PDG in the scalar isosinglet (IJPC=00++) channel in the energy region up to  ≃  2 GeV: f0(500)/σ, f0(980), f0(1370), f0(1500), f0(1710), f0(2020) and f0(2100). The last two are termed unestablished [5]; the others have been subject of various studies in the last decades [10, 11, 1552, 82, 94]. As mentioned in the Introduction, the general conclusion is that the states up to and including f0(1710) are compatible with having ground-state q¯q or q¯q¯qq structure; the presence of the scalar glueball is also expected [42, 5372, 83, 95]. However, none of these states is considered as the first radial excitation of the scalar isosinglet q¯q state.A decade ago, a new resonance named f0(1790) was observed by the BES II Collaboration in the ππ final states produced in J radiative decays [131]; there had been evidence for this state in the earlier data of MARK III [185] and BES [186]. Recently, LHCb has confirmed this finding in a study of Bs → Jππ decays [132]. Since, as indicated, the spectrum of ground-state scalar quarkonia appears to be contained in the already established resonances, we will work here with the hypothesis that f0(1790) is the first excitation of the n¯n ground state (σNE). The assignment is further motivated by the predominant coupling of f0(1790) to pions [131]. The data of Ref. [131] will be used as follows: mf0(1790) = (1790 ± 35) MeV and Γf0(1790)→ππ = (270 ± 45) MeV, with both errors made symmetric and given as arithmetic means of those published by BES II. Additionally, Ref. [131] also reports the branching ratios J/Ψ → ϕf0(1790) → ϕππ = (6.2 ± 1.4) · 10-4 and J/Ψ → ϕf0(1790) → ϕKK = (1.6 ± 0.8) · 10-4. Using Γf0(1790)→ππ = (270 ± 45) MeV and the quotient of the mentioned branching ratios we estimate Γf0(1790)→KK = (70 ± 40) MeV. These data will become necessary in Sects. 3.2 and 3.3. We note, however, already at this point that the large uncertainties in f0(1790) decays – a direct consequence of uncertainties in the J branching ratios amounting to  ∼ 23% and 50% – will lead to ambiguities in prediction of some decays (see Sect. 3.3.1). These are nonetheless the most comprehensive data available at the moment, and more data would obviously be of great importance. The assignment of our excited isoscalar s¯s state σSE will be discussed as a consequence of the model [particularly in the context of f0(2020) and f0(2100)].
  • Two resonances are denoted as established by the PDG in the IJPC = 10++ channel: a0(980) and a0(1450) [5]. Various interpretations of these two states in terms of ground-state q¯q or q¯q¯qq structures or meson–meson molecules have been proposed [20, 23, 24, 26, 28, 3032, 3641, 43, 49, 52, 73, 74, 76].Recently, the BABAR Collaboration [187] has claimed the observation of a new resonance denoted a0(1950) in the process γγηc(1S)K¯Kπ with significance up to 4.2 σ. There was earlier evidence for this state in the Crystal Barrel data [188, 189]; see also Refs. [190, 191]. We will discuss the possible interpretation of this resonance in terms of the first IJPC = 10++excitation as a result of our calculations.
  • Two resonances are candidates for the ground-state q¯q resonance in the scalar-kaon channel (with alternative interpretations – just as in the case of the a0 resonances – in terms of q¯q¯qq structures or meson–meson molecules): K0(800)/κ and K0(1430); controversy still surrounds the first of these states [11, 20, 26, 28, 3032, 34, 35, 37, 39, 49, 7476]. A possibility is that K0(1950), the highest-lying resonance in this channel, represents the first excitation, although the state is (currently) unestablished [5]. This will be discussed as a result of our calculations later on.
  • The pseudoscalar isosinglet (IJPC=00-+) channel has six known resonances in the energy region below 2 GeV according to the PDG [5]: η, η(958), η(1295), η(1405), η(1475) and η(1760). Not all of them are without controversy: for example, the observation of η(1405) and η(1475) as two different states was reported by E769 [192], E852 [193], MARK III [194], DM2 [195] and OBELIX [196, 197], while they were claimed to represent a single state named η(1440) by the Crystal Ball [198] and BES [199, 200] Collaborations. It is important to note that a clear identification of pseudoscalar resonance(s) in the energy region between 1.4 GeV and 1.5 GeV depends strongly on a proper consideration, among other, of the KK threshold opening (mKmK = 1385 MeV) and of the existence of the IJPC = 01++ state f1(1420) whose partial wave is known to influence the pseudoscalar one in experimental analyses (see, e.g., Ref. [193]). A comprehensive study of BES II data in Ref. [201], which included an energy-dependent Breit–Wigner amplitude as well as a dispersive correction to the Breit–Wigner denominator (made necessary by the proximity to the KK threshold), has observed only a marginal increase in fit quality when two pseudoscalars are considered. In line with this, our study will assume the existence of η(1440) to which our ηSE state will be assigned. We will use mη(1440) = (1432 ± 10) MeV and Γη(1440)→KK = (26 ± 3) MeV [199, 200] in Sects. 3.2 and 3.3.2; the error in the decay width is our estimate. We emphasise, however, that our results are stable up to a  ≲ 3% change when η(1475) is considered instead of η(1440).2 Our state ηNE will be assigned to η(1295) in order to test the hypothesis whether an excited pseudoscalar isosinglet at  ≃ 1.3 GeV can be accommodated in eLSM (and notwithstanding the experimental concerns raised in Ref. [203]). We will use the PDG value mη(1295) = (1294 ± 4) MeV for determination of mass parameters in Sect. 3.2. The PDG also reports Γη(1295)total=(55±5) MeV; the relative contributions of η(1295) decay channels are uncertain. Nonetheless, we will use Γη(1295)total in Sect. 3.3.2.
  • Two states have the quantum number of a pion excitation: π(1300) and π(1800), with the latter being a candidate for a non-q¯q state [5]. The remaining π(1300) resonance may in principle be an excited q¯q isotriplet; however, due to the experimental uncertainties reported by the PDG [mπ(1300) = (1300 ± 100) MeV but merely an interval for Γπ(1300) = (200 - 600) MeV] this will only be discussed as a possible result of our model.
  • Two states are candidates for the excited kaon: K(1460) and K(1830). Since other excited states of our model have been assigned to resonances with energies  ≃ 1.4 GeV, we will study the possibility that our IJP = ½0- state corresponds to K(1460). This will, however, only be discussed as a possible result of the model since the experimental data on this state is very limited: mK(1460) ∼ 1460 MeV; ΓK(1460) ∼ 260 MeV [5].

As indicated in the above points, with regard to the use of the above data for parameter determination we exclude as input all states for which there are only scarce/unestablished data and, additionally, those for which the PDG cites only intervals for mass/decay width (since the latter lead to weak parameter constraints). Then we are left with only three resonances whose experimental data shall be used: f0(1790), η(1295) and η(1440). For clarity, we collect the assignment of the model states (where possible), and also the data that we will use, in Table Table2.2. The data are used in Sect. 3.

Table 2
Assignment of the states in Eq. (17) to physical states. Every assignment implies the hypothesis that the physical state has the q¯q structure

Parameters

The following parameters are present in Eq. (16):

g1E,α,m0,λ0,λ1,2,κ1,2,3,4,ξ1,2,3,4,ϵSE,c1,c1E,h1,2,3,h1,2,3E.
19

The number of parameters relevant for masses and decays of the excited states is significantly smaller as apparent once the following selection criteria are applied:

  • All large-Nc suppressed parameters are set to zero since their influence on the general phenomenology is expected to be small and the current experimental uncertainties do not permit their determination. Hence the parameters λ1, h1 and κ1,2,3,4 are discarded.
  • The parameter c1 is set to zero since it contains a term  ∼ (detΦ)2, which would influence ground-state mass terms after condensation of σN and σS. Such introduction of an additional parameter is not necessary since, as demonstrated in Ref. [94], the ground states are very well described by Lagrangian (3).
  • As a first approximation, we will discard all parameters that lead to particle mixing and study whether the assignments described in Table Table22 are compatible with experiment. Hence we discard the parameters α, λ0 and ξ1; note that mixing is also induced by κ1,2 and c1 but these have already been discarded for reasons stated above.3
  • Parameters that lead to decays with two or more excited final states are not of relevance for us: all states in the model have masses between  ∼ 1 GeV and  ∼ 2 GeV and hence such decays are kinematically forbidden. (Parameters λ2 and ξ2 that contribute to mass terms are obviously relevant and excepted from this criterion.) Hence we can discard ξ3,4, c1E and h1,2,3E.

Note that the above criteria are not mutually exclusive: some parameters may be set to zero on several grounds, such as for example κ1.

Consequently we are left with the following undetermined parameters:

g1E,m0,λ2,ξ2,ϵSE,h2,3.
20

The number of parameters that we will actually use is even smaller, as we discuss in Sects. 2.3.3 and 2.3.4.

Mass terms

The following mass terms are obtained for the excited states present in the model:

mσNE2=(m0)2+λ2+ξ22ϕN2,
21

ma0E2=(m0)2+λ2+ξ22ϕN2,
22

mπE2=mηNE2=(m0)2+λ2-ξ22ϕN2,
23

mηSE2=(m0)2-2ϵSE+λ2-ξ2ϕS2
24

mσSE2=(m0)2-2ϵSE+λ2+ξ2ϕS2,
25

mKE2=(m0)2-ϵSE+λ24ϕN2-ξ22ϕNϕS+λ22ϕS2,
26

mK0E2=(m0)2-ϵSE+λ24ϕN2+ξ22ϕNϕS+λ22ϕS2.
27

The mass terms (21)–(27) contain the same linear combination of m0 and λ2:

C1=(m0)2+λ22ϕN2,
28

and the mass terms (24)–(27) contain the same linear combination of λ2 and ϵSE:

C2=λ2ZKfK(ZKfK-ϕN)-ϵSE.
29

This is obvious after substituting the strange condensate ϕS by the non-strange condensate ϕN via Eq. (15). The modified mass terms then read

mσNE2=C1+ξ22ϕN2,
30

ma0E2=C1+ξ22ϕN2,
31

mπE2=mηNE2=C1-ξ22ϕN2,
32

mηSE2=C1+2C2-ξ22(ϕN-2ZKfK)2,
33

mσSE2=C1+2C2+ξ22(ϕN-2ZKfK)2,
34

mKE2=C1+C2+ξ22ϕN(ϕN-2ZKfK),
35

mK0E2=C1+C2-ξ22ϕN(ϕN-2ZKfK).
36

Mass terms for all eight excited states can hence be described in terms of only three parameters from Eq. (16): C1, C2 and ξ2.

Decay widths

Our objective is to perform a tree-level calculation of all kinematically allowed two- and three-body decays for all excited states present in the model. The corresponding interaction Lagrangians are presented in Appendix A. As we will see, there are more than 35 decays that can be determined in this way but all of them can be calculated using only a few formulae.

The generic formula for the decay width of particle A into particles B and C reads

ΓABC=I|k|8πmA2MABC2,
37

where k is the three-momentum of one of the final states in the rest frame of A and is the decay amplitude (i.e., a transition matrix element). is a symmetry factor emerging from the isospin symmetry – it is determined by the number of sub-channels for a given set of final states (e.g., = 2 if B and C both correspond to kaons). Usual symmetry factors are included if the final states are identical. As we will see in Sect. 3.3, decay widths obtained in the model are generally much smaller than resonance masses; for this reason, we do not expect large unitarisation effects [96].

Depending on the final states, the interaction Lagrangians presented in Appendix A can have one of the following general structures:

  • For a decay of the form S → P1P2, where S is a scalar and P1 and P2 are pseudoscalar particles, the generic structure of the interaction Lagrangian is
    LSP1P2=DSP1P2SP1P2+ESP1P2SμP1μP2+FSP1P2μSμP1P2,
    38
    where DSP1P2, ESP1P2 and FSP1P2 are combinations of (some of the) parameters entering Lagrangian (16). According to Eq. (37), the decay width reads in this case
    ΓSP1P2=I|k|8πmS2|DSP1P2-ESP1P2K1·K2+FSP1P2K·K1|2,
    39
    where K, K1 and K2 are respectively 4-momenta of S, P1 and P2.
  • For a decay of the form S → VP, where V is a vector and P is a pseudoscalar particle, the generic structure of the interaction Lagrangian is
    SVPDSVP SVμμP
    40
    where DSVP is a combination of (some of the) parameters entering Lagrangian (16). The decay width reads in this case
    ΓSVP=I|k|8πmS2DSVP2×(mS2-mV2-mP2)24mV2-mP2.
    41
  • For a decay of the form S → V1V2, where V1 and V2 are vector particles, the generic structure of the interaction Lagrangian is
    LSV1V2=DSV1V2SV1μV2μ,
    42
    where DSV1V2 is a combination of (some of the) parameters entering Lagrangian (16). Then the decay width reads
    ΓSV1V2=I|k|4πmS2DSV1V22×(mS2-mV12-mV22)28mV12mV22+1.
    43

As is evident from Appendix A, the most general interaction Lagrangian for 3-body decays of the form S → S1S2S3 is

LSS1S2S3=DSS1S2S3SS1S2S3+ESS1S2S3S(μS1μS2)S3+(analogous terms with derivative couplingsamong final states only).
44

The ensuing formula for the decay width reads

ΓSS1S2S3=I132(2π)3mS3(mS1+mS2)2(mS-mS3)2×dm122(m23)min.(m23)max.dm232MSS1S2S32
45

where m122=(KS1+KS2)2, m232=(KS2+KS3)2 and

(m23)min.=(E2+E3)2-(E2)2-mS22+(E3)2-mS322,
46

(m23)max.=(E2+E3)2-(E2)2-mS22-(E3)2-mS322,
47

with

E2=m122-mS12+mS222m12,E3=mS2-m122-mS322m12.
48

As is evident from Appendix A, our decay widths depend on the following parameters: g1E, λ2, ξ2 and h2,3. The first three appear only in decays with an excited final state; since such decays are experimentally unknown, it is not possible to determine these parameters (and ξ2 can be determined from the mass terms in any case; see Sect. 2.3.3). The remaining two, h2,3, can be calculated from decays with ground states in the outgoing channels – we will discuss this in Sect. 3.3.

Masses and decays of the excited states: results and consequences

Parameter determination: general remarks

Combining parameter discussion at the end of Sects. 2.3.3 and 2.3.4, the final conclusion is that the following parameters need to be determined:

C1,C2,ξ2,h2andh3
49

with C1 and C2 parameter combinations defined in Eqs. (28) and (29).

As is evident from mass terms (30)–(36) and Appendix A, C1 and C2 influence only masses; ξ2 appears in decays with one excited final state and in mass terms. Since, as indicated at the end of Sect. 2.3.4, decays with excited final states are experimentall unknown, ξ2 can only be determined from the masses. Contrarily, h2 and h3 appear only in decay widths (with no excited final states). Hence our parameters are divided in two sets, one determined by masses (C1, C2 and ξ2) and another determined by decays (h2 and h3).

Parameter determination will ensue by means of a χ2 fit. Scarcity of experimental data compels us to have an equal number of parameters and experimental data entering the fit; although in that case the equation systems can also be solved exactly, an advantage of the χ2 fit is that error calculation for parameters and observables is then straightforward.

The general structure of the fit function χ2 fit is as follows:

χ2(p1,,pm)=i=1nOith.(p1,,pm)-Oiexp.ΔOiexp.2
50

for a set of n (theoretical) observables Oith. determined by m ≤ n parameters pj. In our case, mn = 3 for masses and mn = 2 for decay widths. Central values and errors on the experimental side are, respectively, denoted Oiexp. and ΔOiexp.. Parameter errors Δpi are calculated as the square roots of the diagonal elements of the inverse Hessian matrix obtained from χ2(pj). Theoretical errors ΔOi for each observable Oi are calculated by diagonalising the Hesse matrix via a special orthogonal matrix M

MHMt ≡ diag{eigenvalues of H}
51

and rotating parameters pi such that

qM(ppmin.)
52

where p contains all parameters and pmin. realises the minimum of χ2(p1, …, pm). Then we can determine ΔOi via

ΔOi=j=1nOi(q1,qm)qjat fit value ofOiΔqj2
53

(see also Chapter 39 of the Particle Data Book [5]).

Masses of the excited states

Following the discussion of the experimental data on excited states in Sect. 2.3.1 and particle assignment in Table Table2,2, we use the following masses for the χ2 fit of Eq. (50): mσNEmf0(1790)=(1790±35) MeV, mηNEmη(1295)=(1294±4) MeV and mηSEmη(1440)=(1432±10) MeV. Results for C1, C2 and ξ2 are

C1=(2.4±0.6)·106[MeV2],C2=(2.5±0.2)·105[MeV2],ξ2=57±5.
54

With these parameters, the general discussion from Sect. 3.1 allows us to immediately predict the masses of σSE, a0E, K0E, πE and KE. They are presented in Table Table33.

Table 3
Masses of the excited states present in the model. Masses marked with an asterisk are used as input. There is mass degeneracy of σNE and a0E because we have discarded large-Nc suppressed parameters in our excited-state Lagrangian (16) – ...

Decays of the excited states

Hypothesis: f0(1790) is an excited q¯q state

We have concluded in Sect. 3.1 that only two parameters are of relevance for all decays predictable in the model: h2 and h3. They can be determined from the data on the f0(1790) resonance discussed in Sect. 2.3.1: Γf0(1790)→ππ = (270 ± 45) MeV and Γf0(1790)→KK = (70 ± 40) MeV [131]. Performing the χ2 fit described in Sect. 3.1 we obtain the following parameter values:

h2=67±63,h3=79±63.
55

Large uncertainties for parameters are a consequence of propagation of the large errors for Γf0(1790)→ππ and particularly for Γf0(1790)→KK. As described in Sect. 2.3.1, Γf0(1790)→KK was obtained as our estimate relying upon J branching ratios reported by BES II [131] that themselves had uncertainties between  ∼ 23 and 50%. We emphasise, however, that such uncertainties do not necessarily have to translate into large errors for the observables. The reason is that error calculation involves derivatives at central values of parameters [see Eq. (53)]; small values of derivatives may then compensate the large parameter uncertainties. This is indeed what we observe for most decays.

There is a large number of decays that can be calculated using the interaction Lagrangians in Appendix A, parameter values in Eq. (55), formulae for decay widths in Eqs. (39), (41), (43) and (45) as well as Eq. (53) for the errors of observables. All results are presented in Table Table44.

Table 4
Decays and masses of the excited q¯q states. Widths marked as “suppressed” depend only on large-Nc suppressed parameters that have been set to zero. Widths marked with an asterisk are used as input; the others are predictions

The consequences of f0(1790) input data are then as follows:

  • The excited states are generally rather narrow with the exception of f0(1790) and η(1440) whose full decay widths, considering the errors, are, respectively, between  ∼ 300 and  ∼ 500 MeV and up to  ∼ 400 MeV. The result for f0(1790) is congruent with the data published by LHCb [132]; the large interval for the η(1440) width is a consequence of parameter uncertainties, induced by ambiguities in the experimental input data.
  • The excited pion and kaon states are also very susceptible to parameter uncertainties that lead to extremely large errors for the πE and KE decay widths [𝒪(1 GeV)]. A definitive statement on these states is therefore not possible. Contrarily, in the case of η(1295), the three decay widths accessible to our model (for ηNEηππ+ηππ+πKK) amount to (7 ± 3) MeV and hence contribute very little to the overall decay width Γη(1295)total=(55±5) MeV.
  • Analogously to the above point, parameter uncertainties also lead to extremely large width intervals for the decays of scalars into vectors. These decays are therefore omitted from Table Table4,4, except for the large-Nc suppressed decays σSEρρ and σSEωω.
  • Notwithstanding the above two points, we are able to predict more than 35 decay widths for all states in our model except πE and KE. The overall correspondence of the model states to the experimental (unconfirmed) ones is generally rather good, although we note that our scalar s¯s state appears to be too narrow to fully accommodate either of the f0(2020) and f0(2100) states. The mass of our isotriplet state a0E is also somewhat smaller than that of a0(1950) – we will come back to this point in Sect. 3.3.3.

Hypothesis: η(1295) and η(1440) are excited q¯q states

As indicated above, results presented in Table Table44 do not allow us to make a definitive statement on all excited pseudoscalars. However, the situation changes if the parameters h2 and h3 are determined with the help of the η(1295) and η(1440) decay widths.

Using ΓηNEηππ+ηππ+πKK=(55±5) MeV [5] and Γη(1440)→KK = 26 ± 3 MeV (from Ref. [199]; our estimate for the error) we obtain

h2=70±2,h3=35±3.
56

The parameters (56) are strongly constrained and there is a very good correspondence of the pseudoscalar decays to the experimental data in this case (see Table Table5).5). Nonetheless, there is a drawback: all scalar states become unobservable due to very broad decays into vectors. Thus comparison of Tables 4 and and55 suggests that there is tension between the simultaneous interpretation of η(1295), π(1300), η(1440) and K(1460) as well as the scalars as excited q¯q states. A possible theoretical reason is that pseudoscalars above 1 GeV may have non-q¯q admixture. Indeed sigma-model studies in Refs. [37, 41, 43, 204208] have concluded that excited pseudoscalars with masses between 1 GeV and 1.5 GeV represent a mixture of q¯q and q¯q¯qq structures. In addition, the flux-tube model of Ref. [202] and a mixing formalism based on the Ward identity in Ref. [209] lead to the conclusion that the pseudoscalar channel around 1.4 GeV is influenced by a glueball contribution. Hence a more complete description of these states would require implementation of mixing scenarios in this channel.4

Table 5
Decays and masses for the case where η(1295) and η(1440) are enforced as excited q¯q states. Widths marked with an asterisk were used as input. Pseudoscalar observables compare fine with experiment but the scalars are unobservable due to extremely ...

Note, however, that the results of Table Table55 depend on the assumption that the total decay width of η(1295) is saturated by the three decay channels accessible to our model (ηππ, ηππ and Kππ). The level of justification for this assumption is currently uncertain [5]. Consequently we will not explore this scenario further.

Is a0(1950) of the BABAR Collaboration an excited q¯q state?

Encouraging results obtained in Sect. 3.3.1, where f0(1790) was assumed to be an excited q¯q state, can be used as a motivation to explore them further. As discussed in Sect. 2.3.1, data analysis published recently by the BABAR Collaboration has found evidence of an isotriplet state a0(1950) with mass ma0(1950) = (1931 ± 26) MeV and decay width Γa0(1950) = (271 ± 40) MeV [187].

Assuming that f0(1790) is an excited q¯q state (as already done in Sect. 3.3.1), we can implement ma0(1950) obtained by BABAR as a large-Nc suppressed effect in our model as follows. Mass terms for excited states σNE and σSE, Eqs. (30) and (34), can be modified by reintroduction of the large-Nc suppressed parameter κ2 and now read

mσNE2=C1+ξ22+2κ2ϕN2,
57

mσSE2=C1+2C2+ξ22+2κ2(ϕN-2ZKfK)2.
58

The other mass terms [Eqs. (31)–(33), (35) and (36)] remain exactly the same; κ2 does not influence any decay widths. We can now repeat the calculations described in Sect. 3.2 with the addition that the mass of our state a0E corresponds exactly to that of a0(1950). We obtain

C1=(2.4±0.6)·106[MeV2],C2=(2.5±0.2)·105[MeV2],ξ2=57±5,κ2=-10±3.
59

Note that a non-vanishing value of κ2 introduces mixing of σNE and σSE in our Lagrangian (16). Its effect is, however, vanishingly small since the mixing angle is  ∼ 11.

Using the mass parameters (59) and the decay parameters (55) we can repeat the calculations of Sect. 3.3.1. Then our final results for the mass spectrum are presented in Fig. Fig.11 and for the decays in Table Table6.6. The values of ma0E, mσSE and mK0E have changed in comparison to Table Table44 inducing an increased phase space. For this reason, the decay widths of the corresponding resonances have changed as well. All other results from Table Table44 have remained the same and are again included for clarity and convenience of the reader.

Fig. 1
Masses of excited q¯q states with isospin I, total spin J and parity P from the Extended Linear Sigma Model (left) and masses from the experimental data (right). Area thickness corresponds to mass uncertainties on both panels. The lower 00+( ...
Table 6
Final results: decays and masses of the excited q¯q states. Widths marked as “suppressed” depend only on large-Nc suppressed parameters that have been set to zero. Masses/widths marked with (*) are used as input; others are predictions ...

The consequences are as follows:

  • The decay width of a0E is now Γa0E=(280±90) MeV; it overlaps fully with Γa0(1950) = (271 ± 40) MeV measured by BABAR. Hence, if a0(1950) is confirmed in future measurements, it will represent a very good candidate for the excited isotriplet n¯n state.
  • The mass of σSE is between those of f0(2020) and f0(2100). Judging by the quantum numbers, either of these resonances could represent a (predominant) s¯s state; an option is also that the excited s¯s state with IJPC=00++ has not yet been observed in this energy region. However, one must also remember the possibility that q¯q–glueball mixing (neglected here) may change masses as well as decay patterns. The decay width of σSE is rather narrow (up to 110 MeV) but this may change if mixing effects happen to be large.
  • The mass of K0E is qualitatively (within  ∼  100 MeV) congruent with that of K0(1950); the widths overlap within 1 σ. Hence, if K0(1950) is confirmed in future measurements, it will represent a very good candidate for the excited scalar kaon.
  • Conclusions for all other states remain as in Sect. 3.3.1.

Conclusion

We have studied masses and decays of excited scalar and pseudoscalar q¯q states (quds quarks) in the Extended Linear Sigma Model (eLSM) that, in addition, contains ground-state scalar, pseudoscalar, vector and axial-vector mesons.

Our main objective was to study the assumption that the f0(1790) resonance is an excited n¯n state. This assignment was motivated by the observation in BES [131] and LHCb [132] data that the resonance couples mostly to pions and by the theoretical statement that the n¯n ground state is contained in the physical spectrum below f0(1790). Furthermore, the assumption was also tested that the a0(1950) resonance, whose discovery was recently claimed by the BABAR Collaboration [187], represents the isotriplet partner of f0(1790).

Using the mass, 2π and 2K decay widths of f0(1790), the mass of a0(1950) and the masses of the pseudoscalar isosinglets η(1295) and η(1440) our model predicts more than 35 decays for all excited states except for the excited pion and kaon (where extremely large uncertainties are present due to experimental ambiguities). All numbers are collected in Table Table66.

In essence: the f0(1790) resonance emerges as the broadest excited q¯q state in the scalar channel with Γf0(1790) = (405 ± 96) MeV; a0(1950), if confirmed, represents a very good candidate for the excited q¯q state; K0(1950), if confirmed, represents a very good candidate for the excited scalar kaon.

Our excited isoscalar s¯s state has a mass of (2038 ± 24) MeV, placed between the masses of the nearby f0(2020) and f0(2100) resonances; also, its width is relatively small ( ≤ 110 MeV). We conclude that, although any of these resonances may in principle represent a q¯q state, the introduction of mixing effects (particularly with a glueball state) may be necessary to further elucidate their structure.

Our results also imply a quite small contribution of the ηππ, ηππ and πKK decays to the overall width of η(1295). For η(1440), the decay width is compatible with any value up to  ∼ 400 MeV (ambiguities due to uncertainty in experimental input data).

It is also possible to implement Γη(1295)totalΓη(1295)ηππ+ηππ+πKK and Γη(1440)→KK exactly as in the data of PDG [5] and BES [199]. Then π(1300) and K(1460) are quite well described as excited q¯q states – but the scalars are unobservably broad (see Table Table5).5). Hence, in this case, there appears to be tension between the simultaneous description of η(1295), π(1300), η(1440) and K(1460) and their scalar counterparts as excited q¯q states. This scenario is, however, marred by experimental uncertainties: for example, it is not at all clear if the width of η(1295) is indeed saturated by the ηππ, ηππ and πKK decays. It could therefore only be explored further when (very much needed) new experimental data arrives – from BABAR, BES, LHCb or PANDA [81] and NICA [212].

Acknowledgements

We are grateful to D. Bugg, C. Fischer and A. Rebhan for extensive discussions. The collaboration with Stephan Hübsch within a Project Work at TU Wien is also gratefully acknowledged. The work of D. P. is supported by the Austrian Science Fund FWF, Project No. P26366. The work of F. G. is supported by the Polish National Science Centre NCN through the OPUS project nr. 2015/17/B/ST2/01625.

Appendix A: Interaction Lagrangians

Here we collect all interaction Lagrangians that are used for calculations of decay widths throughout this article. Vertices for large-Nc suppressed decays are not included but briefly discussed after each Lagrangian in which they appear.

Appendix A.1: Lagrangian for σNE

The Lagrangian reads

LσNE=12(h2-h3)wa12Zπ2ϕNσNE(μηN)2+(μπ)2+12h2ϕN-2h3ϕSwK12ZK2σNE×μK¯0μK0+μK-μK++(h2-h3)wa1ZπϕNσNEf1NμμηN+a1μ·μπ+12h2ϕN-2h3ϕSwK1ZKσNE×K¯1μ0μK0+K1μ-μK++ h.c.+12(h2+h3)ϕNσNE(ωNμ)2+(ρμ)2+12h2ϕN+2h3ϕSσNEK¯μ0Kμ0+Kμ-Kμ+-ξ2ZπϕNσNEπE·π-g1Ewa1ZπσNEμπE·μπ+12(h2-h3)wa12Zπ2σNEσN(μπ)2.
A.1

Note: the decay σNEηSηS ( ∼ κ1, h1) is large-Nc suppressed.

Appendix A.2: Lagrangian for σSE

The Lagrangian reads

LσSE=(h2-h3)wf1S2ZηS2ϕSσSE(μηS)2+h2ϕS-h32ϕN×wK12ZK2σSEμK¯0μK0+μK-μK++h2ϕS-h32ϕNwK1ZKσSE×K¯1μ0μK0+K1μ-μK++ h.c.+h2ϕS+h32ϕNσSEK¯μ0Kμ0+Kμ-Kμ+.
A.2

Note: the decays σSEππ ( ∼ κ1, h1), σSEηNηN ( ∼ κ1, h1), σSEρρ (h1), σSEωNωN (h1), σSEa1π (h1), σSEf1NηN (h1), σSEπEπ ( ∼ κ2), σSEηNEηN ( ∼ κ2) and σSEσSππ ( ∼ κ1, h1) are large-Nc suppressed.

Appendix A.3: Lagrangian for a0E

The Lagrangian reads (only a00E included; decays of a0±E follow from isospin symmetry):

La0E=(h2-h3)wa12Zπ2ϕNa00Eμπ0μηN-12h2ϕN-2h3ϕSwK12ZK2a00E×μK¯0μK0-μK-μK++(h2-h3)wa1ZπϕNa00Ef1Nμμπ0+a1μ0μηN-12h2ϕN-2h3ϕSwK1ZKa00E×K¯1μ0μK0-K1μ-μK++ h.c.+(h2+h3)ϕNa00Eρμ0ωNμ-12h2ϕN+2h3ϕS×a00EK¯μ0Kμ0-Kμ-Kμ+-ξ2ZπϕNa00EηNEπ0-g1Ewa1Zπa00EμηNEμπ0+12(h2+h3)wa12Zπ2a00Ea00(μπ)2-h3wa12Zπ2a00Eμπ0a0·μπ.
A.3

Appendix A.4: Lagrangian for K0E

The Lagrangian reads (only K00E included; decays of other K0E components follow from isospin symmetry):

LK0E=14h2ϕN+2ϕS-2h3ϕNwa1wK1ZπZKK00E×μK¯0μηN-μK¯0μπ0+2μK-μπ++122h2ϕN+2ϕS-22h3ϕS×wf1SwK1ZηSZKK00EμK¯0μηS+14h2ϕN+2ϕS-2h3ϕNwK1ZKK00E×f1NμμK¯0-a1μ0μK¯0+2a1μ+μK-+14h2ϕN+2ϕS-2h3ϕNwa1ZπK00E×K¯1μ0μηN-K¯1μ0μπ0+2K1μ-μπ++122h2ϕN+2ϕS-22h3ϕSwf1SZηSK00EK¯1μ0μηS+14h2ϕN+2ϕS+2h3ϕNK00E×K¯μ0ωNμ-K¯μ0ρμ0+2Kμ-ρμ+-142ξ2ϕN-λ2ϕN-2ϕSZKK00E×K¯0ηNE-K¯0π0E+2K-π+E-12g1EwK1ZKK00E×μK¯0μηNE-μK¯0μπ0E+2μK-μπ+E+12g1EwK1ZKμK00E×μK¯0ηNE-μK¯0π0E+2μK-π+E+12ξ2ZπϕSK00EK¯0Eπ0-2K-Eπ++12g1Ewa1ZπK00E×μK¯0Eμπ0-2μK-Eμπ+-12g1Ewa1ZπμK00E×K¯0Eμπ0-2K-Eμπ++14h2wa12Zπ2ZKSK00EK¯00(μπ)2+i4(h2-2h3)wa1wKZπ2ZKSK00Eπ0μK¯00μπ0-ih3wa1wKZπ2ZKSK00Eπ-μK¯00μπ++i2h2wa1wKZπ2ZKSK00Eπ+μK¯00μπ-+i22(h2+2h3)wa1wKZπ2ZKSK00E×π+μK0-μπ0-π0μK0-μπ+.
A.4

Appendix A.5: Lagrangian for ηNE

Only three-body decays into pseudoscalars are kinematically allowed for this particle:

LηNE=12(h2-h3)wa12Zπ3ηNEηN(μπ)2+(h2-h3)wa12Zπ3ηNEμηNμπ·π-14(h2-2h3)wa1wK1ZπZK2ηNE×K¯0μK0μπ0-2K¯0μK+μπ--K-μK+μπ0-2K-μK0μπ++ h.c.-12h2wK12ZπZK2ηNE×π0μK¯0μK0-π0μK-μK+-2π-μK+μK¯0+ h.c..
A.5

Appendix A.6: Lagrangian for ηSE

The Lagrangian reads

LηSE=-i2h3wK1ZKϕNηSEμK¯0Kμ0+μK-Kμ++ h.c.+(h2-h3)wa12Zπ3ηNEμηNμπ·π-122h2wa1wK1ZπZK2ηSEK¯0μK0μπ0-2K¯0μK+μπ--K-μK+μπ0-2K-μK0μπ++ h.c.+12h3wK12ZπZK2ηSE×π0μK¯0μK0+π0μK-μK++2π-μK+μK¯0+ h.c..
A.6

Note: the decay ηSEηSππ ( ∼ κ1, h1) is large-Nc suppressed.

Appendix A.7: Lagrangian for πE

The Lagrangian reads (only π0E included; decays of π±E follow from isospin symmetry):

LπE=-ih3wa1ZπϕNπ0Eρμ-μπ+-ρμ+μπ-+14h2-2h3wa1wK1ZπZK2π0Eμπ0×K¯0μK0+K-μK++ h.c.+12h2wK12ZπZK2π0Eπ0μK¯0μK0+μK-μK+-122h2+2h3wa1wK1ZπZK2π0E×μπ-K¯0μK+-K+μK¯0+ h.c.+12(h2+h3)wa12Zπ3π0Eπ0(μπ)2-h3wa12Zπ3π0Eμπ0π·μπ.
A.7

Appendix A.8: Lagrangian for KE

The Lagrangian reads (only K0E included; decays of other KE components follow from isospin symmetry):

LKE=-i4h2ϕN-2ϕS+2h3ϕNwK1ZKK0E×ωNμμK¯0-ρμ0μK¯0+2ρμ+μK--i4h2ϕN-2ϕS-2h3ϕNwa1ZπK0E×K¯μ0μηN-K¯μ0μπ0+2Kμ-μπ+-i22h2ϕN-2ϕS+22h3ϕS×wf1SZηSK0EK¯μ0μηS-12h2wa12Zπ2ZKK0EK¯0μηNμπ0-2K-μηNμπ+-14(h2-2h3)wa1wK1Zπ2ZKK0Eπ0μηNμK¯0-2π+μηNμK-+ηNμπ0μK¯0-2ηNμπ+μK-+12h3wa1wf1SZπZKZηSK0E×K¯0μηSμπ0-2K-μηSμπ+-122h2wK1wf1SZπZKZηSK0E×π0μηSμK¯0-2π+μηSμK--122h2wa1wK1ZπZKZηSK0E×ηSμπ0μK¯0-2ηSμπ+μK-+14h2wa12Zπ2ZKK0EK¯0(μπ)2+14(h2-2h3)×wa1wK1Zπ2ZKK0Eπ0μK¯0μπ0-h3wa1wK1Zπ2ZKK0Eπ-μK¯0μπ++12h2×wa1wK1Zπ2ZKK0Eπ+μK¯0μπ-+122(h2+2h3)wa1wK1Zπ2ZKK0E×π+μK-μπ0-π0μK-μπ+.
A.8

Footnotes

1There is a subtle point pertaining to the condensation of excited states in σ-type models: as discussed in Ref. [184], it can be in agreement with QCD constraints but may also, depending on parameter choice, spontaneously break parity in vacuum. Study of a model with condensation of the excited states would go beyond the current work. (It would additionally imply that the excited pseudoscalars also represent Goldstone bosons of QCD which is disputed in, e.g., Ref. [111].)

2The η(1405) resonance would then be a candidate for the pseudoscalar glueball [202].

3However, there would be no mixing of pseudoscalar isosinglets ηNE and ηSE in the model even if all discarded parameters were considered. The reason is that there is no condensation of excited scalar states in Lagrangian (16).

4A similar mixing scenario may (as a matter of principle) also exist in the case of the scalars discussed here. However, the amount of theoretical studies is significantly smaller here: for example, a glueball contribution to f0(1790) has been discussed in Refs. [210, 211] while – just as in our study – the same resonance was found to be compatible with an excited q¯q state in Ref. [102].

Contributor Information

Denis Parganlija, ta.ca.neiwut.pti.peh@psined, http://hep.itp.tuwien.ac.at/~denisp/

Francesco Giacosa, lp.ude.kju@asocaigf, http://www.ujk.edu.pl/strony/Francesco.Giacosa/

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