Issue 
A&A
Volume 607, November 2017



Article Number  A108  
Number of page(s)  11  
Section  Extragalactic astronomy  
DOI  https://doi.org/10.1051/00046361/201630069  
Published online  22 November 2017 
Galaxy clusters in the context of superfluid dark matter
^{1} School of Physics and Astronomy, University of St. Andrews, St. Andrews, KY16 9SS, UK
email: aoh2@standrews.ac.uk
^{2} Center for Particle Cosmology, Department of Physics and Astronomy, University of Pennsylvania, Philadelphia, PA 19104, USA
^{3} Université de Strasbourg, CNRS UMR 7550, Observatoire Astronomique de Strasbourg, 11 rue de l’Université, 67000 Strasbourg, France
Received: 15 November 2016
Accepted: 20 July 2017
Context. The mass discrepancy in the Universe has not been solved by the cold dark matter (CDM) or the modified Newtonian dynamics (MOND) paradigms so far. The problems and solutions of either scenario are mutually exclusive on large and small scales. It has recently been proposed, by assuming that dark matter is a superfluid, that MONDlike effects can be achieved on small scales whilst preserving the success of ΛCDM on large scales. Detailed models within this “superfluid dark matter” (SfDM) paradigm are yet to be constructed.
Aims. Here, we aim to provide the first set of spherical models of galaxy clusters in the context of SfDM. We aim to determine whether the superfluid formulation is indeed sufficient to explain the mass discrepancy in galaxy clusters.
Methods. The SfDM model is defined by two parameters. Λ can be thought of as a mass scale in the Lagrangian of the scalar field that effectively describes the phonons, and it acts as a coupling constant between the phonons and baryons. m is the mass of the DM particles. Based on these parameters, we outline the theoretical structure of the superfluid core and the surrounding “normalphase” dark halo of quasiparticles. The latter are thought to encompass the largest part of galaxy clusters. Here, we set the SfDM transition at the radius where the density and pressure of the superfluid and normal phase coincide, neglecting the effect of phonons in the superfluid core. We then apply the formalism to a sample of galaxy clusters, and directly compare the SfDM predicted mass profiles to data.
Results. We find that the superfluid formulation can reproduce the Xray dynamical mass profile of clusters reasonably well, but with a slight underprediction of the gravity in the central regions. This might be partly related to our neglecting of the effect of phonons in these regions. Two normalphase halo profiles are tested, and it is found that clusters are better defined by a normalphase halo resembling an NavarroFrenkWhitelike structure than an isothermal profile.
Conclusions. In this first exploratory work on the topic, we conclude that depending on the amount of baryons present in the central galaxy and on the actual effect of phonons in the inner regions, this superfluid formulation could be successful in describing galaxy clusters. In the future, our model could be made more realistic by exploring nonsphericity and a more realistic SfDM to normal phase transition. The main result of this study is an estimate of the order of magnitude of the theory parameters for the superfluid formalism to be reasonably consistent with clusters. These values will have to be compared to the true values needed in galaxies.
Key words: Xrays: galaxies: clusters / dark matter / galaxies: kinematics and dynamics / galaxies: clusters: general / cosmology: miscellaneous
© ESO, 2017
1. Introduction
While observations of largescale structure in the Universe are traditionally explained by invoking a nonuniform distribution of dark matter (DM) particles, the nature of such particles and the strength of their interactions so far remain unknown. Such particles might be of any type as long as they are collisionfree nonrelativistic massive particles on scales of galaxy clusters and above, as in the standard ΛCDM paradigm. A strong argument for the existence of such particles is the colliding bullet cluster (Clowe et al. 2006), which has a lensing signature offset from its baryonic centre. This is explained in the cold dark matter (CDM) paradigm, as the gas of the cluster interacts while CDM does not, and thus the gas stays closer to the centre and the dark matter can pass through almost unaffected. This therefore produces the observed lensing signature of the bullet cluster.
Until DM particles are directly detected, it is useful, however, to keep in mind that its properties could be more complex than currently envisaged (e.g. Lee 2016; Hui et al. 2017). For instance, on small scales, there are still some issues with interactionfree particle models, especially to explain the dynamics of galaxies. The most widely discussed problems are the cuspcore problem, the missing satellites problem, the toobigtofail problem, and satellite plane problems (e.g. Walker & Peñarrubia 2011; Dubinski & Carlberg 1991; de Blok 2010; Klypin et al. 1999; Moore et al. 1999; BoylanKolchin et al. 2012, 2011; Ibata et al. 2013; Pawlowski et al. 2015). These open questions have led a part of the community to search for an alternative to the CDM paradigm to explain the observed dynamics of galaxies. The general problem of CDM in galaxies indeed seems to be more profound than the series of problems listed above. In particular, a diversity of shapes of rotation curves at a given maximum circular velocity scale are observed, which is contrary to CDM expectations (Oman et al. 2015), and a uniformity of shapes exists at a given baryonic surface density scale (Famaey & McGaugh 2012). These puzzling observations can be summarised by the radial acceleration relation (McGaugh et al. 2016), which is equivalent to the wellknown modified Newtonian dynamics (or MOND) phenomenology for isolated rotationally supported systems (Milgrom 1983a,b,c; Bekenstein & Milgrom 1984; Famaey & McGaugh 2012). The idea of MOND was to introduce an acceleration scale a_{0} in the dynamics, directly illustrating the role that is played by the baryonic surface density in observations. When the gravitational acceleration is much higher than a_{0}, the gravity behaves as Newton predicts. Much below a_{0}, the force law of gravity effectively switches to a force law proportional to 1 /r (instead of Newton’s 1 /r^{2} law). This is also the actual phenomenology of the radial acceleration relation, or mass discrepancy acceleration relation (MDAR). The recent study of Di Cintio & Lelli (2016) aims to determine whether the MDAR can be naturally predicted by ΛCDM. It was found that with a massdependent DM profile, the MDAR can be reproduced, but a universal NavarroFrenkWhite (NFW) profile does not work well in systems below M_{⋆} ≈ 10^{9.5}M_{⊙}.Other studies of this problem found that ΛCDM was able to predict the general trend of the MDAR (Keller & Wadsley 2017; Navarro et al. 2017; Ludlow et al. 2017), but whether the observed scatter and normalisation can be precisely reproduced is still fiercely debated (Desmond 2017; Lelli et al. 2016). On the other hand, a very small scatter would be expected in MOND by construction. However, the MOND phenomenology fails on large scales, for example, galaxy clusters (see for example Sanders 1999), although work has been conducted to reconcile this problem by including neutrinos (e.g. Sanders 2003; Angus et al. 2008; Angus 2009) or by modifying the MOND formulation itself (Zhao & Famaey 2012; Hodson & Zhao 2017a,b).
In short, ΛCDM is successful on large scales, but still has some currently debated problems on small (galactic and subgalactic) scales, whilst MOND seems to have the exact opposite problem. It is therefore interesting to ask the question whether we can have MOND behaviour on small scales and CDMlike behaviour on larger scales. Following up on previous proposals by Blanchet & Heisenberg (2015), for instance, this is exactly what Khoury and Berezhiani recently explored in a series of papers (Berezhiani & Khoury 2015, 2016; Khoury 2016). The idea expressed in these works is the concept that DM behaves like a superfluid in cold enough and dense enough environments, typically within galaxies, and it behaves like normal particle DM (“normal phase”) in clusters and on larger scales. This framework aims to describe the rotation curve in galaxies through a MONDlike phononmediated force resulting from DM when it is in its superfluid phase. In galaxy clusters, however, most of the matter is outside the superfluid phase and is made of quasiparticles in thermal equilibrium.
Each paper discussed a different approach to achieve the desired effect, and we focus here on Berezhiani & Khoury (2015, 2016). These two papers prescribe the fundamental components to the theory, but attempts to make a detailed model of an astrophysical system are lacking so far. Further to the work in these two papers, we must also address how to model the normal phase of the matter and how that embeds the superfluid. In a first attempt to do this, we consider the case of spherical galaxy clusters. The reasons for first choosing galaxy clusters instead of galaxies are that galaxy clusters are commonly modelled in spherical symmetry without the need for a disk component, and very little contribution from the phonon force is therefore expected.
Section 2 outlines how we modelled the dark matter, and we describe the superfluid phase, the normal phase, the transition of one phase transitions to the other, and the determination of the virial mass and radius of the cluster in this context. In Sect. 3 we describe a toy model with no baryons for illustrative purposes. In Sect. 4 we then analyse a sample of galaxy clusters in the context of this model, mainly comparing the derived mass profile of the superfluid to the profile calculated from hydrostatic equilibrium of the gas. We conclude in Sect. 5.
2. Dark matter superfluid model
In this section we give a brief overview of the equations that describe a system in the context of the DM superfluid theory (SfDM). We first recall the general idea of the SfDM model. Ignoring interactions for simplicity, DM particles undergo a phase transition to the superfluid state whenever their de Broglie wavelength λ_{dB} ~ 1 /mv is larger than the average interparticle separation ℓ ~ n^{− 1 / 3}. Here v is typically the DM velocity dispersion, m is the DM particle mass, and n is the local average DM number density. Thus superfluidity arises in sufficiently cold (large λ_{dB}) and dense (small ℓ) environments. Another requirement for BoseEinstein condensation is that DM reaches thermal equilibrium, which requires sufficiently strong selfinteractions (Khoury 2015).
We expect the superfluid phase to be confined within the central regions of clusters, where the density is high enough. Because clusters are hotter than galaxies, most of their DM content should be in the normal phase. The DM in galaxy clusters therefore consists of a superfluid core, whose radius (depending on the theory parameter values) will range fromapproximately 50 to 100 kpc, surrounded by an atmosphere of DM particles in the normal phase. The key element to model here is the transition from one phase to the other. If too large a region in the cluster is in the superfluid phase, it is likely that observed Xray gas temperature profiles cannot be reproduced.
Within the superfluid core, DM is more aptly described as collective excitations, which at low energy are phonons. In the superfluid paradigm of Berezhiani & Khoury (2015, 2016), the MONDlike effects are achieved as a result of phonon excitations in the superfluid phase mediating a longrange force between ordinary matter particles. This phononmediated force is only important at low acceleration (a ≪ a_{0}), resulting in strong deviations from Newtonian gravity. In galaxies, this effect is critical in reproducing the empirical success of MOND at fitting rotation curves. The central regions of galaxy clusters, however, tend to lie in the intermediate (a ~ a_{0}) to Newtonian regime (a ≫ a_{0}), where the phononmediated force is at most comparable to the Newtonian force. We therefore expect that the phonon force is unimportant in galaxy clusters compared to the DM component and therefore, in the interest of simplicity, we assume that the phonon contribution to our calculations is hereafter zero. We stress that this is in no way an acceptable assumption when the internal accelerations are small compared to a_{0}, and thus some of the equations described in the following sections cannot be applied to galaxies. The phonon force must be included for consistency.
2.1. Set up
The gravitational potential Φ is determined as usual by Poisson’s equation, (1)where ρ_{b} and ρ denote the baryon and DM densities, respectively. This allows us to integrate for Φ for any given equation of state ρ(Φ).
For simplicity, we assume hydrostatic equilibrium, which requires (2)where ρ and P are the mass density and pressure of the DM, respectively. This allows us to obtain the pressure everywhere.
In the following, we furthermore assume spherical symmetry, in which case the above equations reduce to (3)and (4)To solve these equations and derive the DM profile in galaxy clusters, multiple parts of the model need to be addressed:

DM superfluid core profile.

DM normal halo profile.

Matching the superfluid core to the normal halo.

Determining the virial radius of the system.

Making total mass the free parameter.
These ingredients are described in turn below.
2.2. Dark matter superfluid core
We begin by reviewing some properties of the inner superfluid core, discussing the pressure, sound speed, gravitational potential, and how they are related.
Ignoring phonons, the pressure of the superfluid is related to its density ρ_{s} via (Berezhiani & Khoury 2015) (5)where Λ is a mass scale and c is the speed of light. We chose Λ to be a mass scale to simplify the units of the Λm^{3} combination that appears throughout. We present Λm^{3} in units of eV^{4}/c^{8}. However, we have made our equations dimensionally sound in real units such that Λ has units of mass, m has units of mass, and ħ has normal units kg m^{2} s^{1}. The superfluid parameters Λ and m always appear in the combination Λm^{3} in our calculations, hence there exists a degeneracy when choosing values. We therefore combine the parameters in this way and only discuss the value of K = Λc^{2}m^{3}/ ħ^{3} in what follows. The degeneracy of the parameter combination Λm^{3} is broken when the phonon force is included. Therefore, as phonons become important on small scales, applying the superfluid paradigm to galaxies will be key in fully understanding these parameters (Berezhiani et al., in prep.).
Equation (5)describes a polytropic equation of state, P ~ ρ^{1 + 1 /n}, with index n = 1 / 2. Substituting the superfluid equation of state in the equation of the hydrostatic equilibrium Eq. (4), we obtain (6)It is easy to see that this is solved by (7)Thus the superfluid density is uniquely specified once we know the gravitational potential. The latter is fixed by integrating Poisson’s equation (Eq. (3)): (8)This can be solved with initial conditions, Φ(r = 0) = Φ_{0} and Φ′(r = 0) = 0, where Φ_{0} is a free parameter to be determined. The central potential gradient should be set in accordance with the baryon potential gradient. However, setting our value to zero did not affect our results. We discuss how we determined this central potential in Sect. 2.7.
The adiabatic sound speed is as usual given by (9)Thus the superfluid sound speed c_{s} is also related to the gravitational potential Φ.
In the absence of baryons (ρ_{b} = 0), Poisson’s Eq. (8) can be cast as a LaneEmden Eq. (Berezhiani & Khoury 2015). The resulting density profile is smooth at the origin and vanishes at a certain radius that defines the core radius. This radius is determined by the parameters of the model (m and Λ) together with the central density. In the presence of baryons, the superfluid profile will of course be altered, but the characteristic feature of a superfluid profile vanishing at a particular radius will remain.
2.3. Dark matter normal halo
2.3.1. Isothermal
The superfluid core is assumed to be surrounded by an atmosphere of normalphase DM particles in thermal equilibrium. For simplicity, we ignore interactions and treat this normal component as an ideal gas, (10)Hydrostatic equilibrium in this case implies the wellknown isothermal profile (11)In the simplified case where we omit the contribution of the baryons, substituting Eq. (11) into the Poisson equation yields the simplified solution (12)The density normalisation ρ_{c} and radius R_{c} are fixed below.
Isothermal DM haloes have an enclosed mass that grows linearly with radius, resulting from the density ρ ∝ r^{2}.
2.3.2. NFW halo
The isothermal case described above is very simple in formulation. For galaxy clusters in ΛCDM, it is common to model haloes using an NFW profile (Navarro et al. 1997; Zhao 1996) which has,at large radius, ρ ∝ r^{3} and a logarithmic mass growth. To mimic this type of behaviour for our normal phase, we tested a density profile of the form (13)Equation (13) has the properties ρ_{n} = ρ_{c} when r = R_{c}, ρ_{n} ∝ r^{1} when r ≪ r_{s}, and ρ_{n} ∝ r^{3} when r ≫ r_{s}.Here the scale radius r_{s} was estimated to closely match NFW profiles for each cluster. For the first toy model examples in Sect. 3 below, we demonstrate the equations with the isothermal profile only for simplicity, but we show the NFW result when analysing the clusters in Sect. 4.
2.4. DM in two phases
Ideally, we would like to build a model with three sections: 1) the inner section, which is dominated by matter in the superfluid phase; 2) the outer halo, which is dominated by normal phase matter; and 3) a transition regime, which has a mixture of normalphase and superfluidphase particles. We neglect this third regime in our model for simplicity and design a system where below the core radius R_{c} only superfluid matter exists, and above R_{c} only normalphase matter is present. The procedure for determining this radius involves continuity of pressure between the two phases of DM and is outlined in Sect. 2.5.
In other words, we modelled the DM in galaxy clusters as a superfluid core (r ≤ R_{c}) with density and pressure ,surrounded by a normal phase of DM in the outer halo (r ≥ R_{c}) with a density profile following Eq. (12) for the isothermal case or Eq. (13) for the NFW case and pressure . The gravitational potential Φ(r) has a meaningful zeropoint fixed by the central density of the superfluid, and K is a constant that is defined in Eq. (5). These two densities are meant to be continuous at the boundary, that is, ρ_{s} = ρ_{n} = ρ_{c} at r = R_{c}, although this boundary condition is independent of the coordinate system and spherical symmetry. These two phases could be continuously interpolated using ρ = ρ_{0}(1−mΦ /k_{B}T/n)^{n}, where in n → 1 / 2 we have the superfluid phase, and in n → ∞ we have the isothermal phase. Alternatively, the real fluid can be thought of as being some superposition of the two fluid phases.
2.5. Matching the superfluid core to the normal halo
As mentioned above, we assumed a model where the superfluid phase abruptly transitions into the normal phase of the fluid. We therefore determined at which radius this transition occurs, which defines the core radius R_{c}. To do this, we imposed the condition that the tangential pressure is continuous at the boundary between the core and normalphase DM. Therefore, the determined radius at which this criterion is satisfied is our core radius R_{c}. We outline this procedure step by step.

Step 1: calculating the gravitational enclosed mass. In order to perform the pressurematching routing, we calculated the total enclosed gravitating mass (baryons + DM) as a function of radius for r ≥ R_{c}: (14)The first term comes from integrating the superfluid density Eq. (7), the second from integrating the normalphase density Eq. (12), and the third is the baryonic mass. We therefore have the enclosed mass as a function of R_{c} and ρ_{c}.

Step 2: solving the Poisson equation. Poisson’s equation (Eq. (8)) is solved numerically given an initial value of the gravitational potential Φ_{0} assuming the central gradient is zero. This yields the gravitational potential profile Φ(r), which can be substituted to obtain the superfluid density profile as explained earlier. In our model, the superfluid density and gravitational potential profiles are only valid for r ≤ R_{c}. The next step is to calculate R_{c}.

Step 3: calculate the core radius: As mentioned, we assumed that the boundary between the normal and superfluid phase of DM is the point at which the tangential pressures are equal. Mathematically, this means the point at which (15)The lefthand side comes from the polytropic equation of state Eq. (5) describing the superfluid, with ρ_{c} = ρ_{s}(R_{c}). The righthand side follows from the hydrostatic equilibrium equation of the normalphase density, where we have substituted Eq. (12) for ρ_{n}(r). Furthermore, M_{grav}(r) refers to the total enclosed mass (baryonic + DM) at radius r. In order to solve Eq. (15) for the core radius R_{c}, we must write the parameters ρ_{c} and M_{grav}(r) as functions of R_{c}. The former is obtained by evaluating Eq. (7) at R_{c}: (16)For the enclosed mass M_{grav}(r), we note that the lower limits of the integral on the righthand side of Eq. (15) are greater than R_{c}, hence we can use our expression Eq. (14), which is valid for r ≥ R_{c}. Therefore by numerically solving Eq. (15) using the derived expressions, for the mass (Eq. (14)) and core density (Eq. (16)) we can determine a value for the core radius, R_{c}. From the calculated core radius, we can find the numerical value for the core density via Eq. (16).
Fig. 1 Toy model of a DMonly system. We highlight the dependence of the superfluid parameters on the choice of virial mass for a system that only includes DM. We stress that this result does not consider baryons, and a more complete analysis should be performed, which we provide for the cluster sample. If we were to include baryons, we would expect to see a slight decrease in core radius for our clusters. This difference would be enhanced in galaxies. Top left: core radius vs. virial mass. Top right: density at the core radius vs. virial mass. Bottom left: central potential vs. virial mass. Bottom right: superfluid core mass vs. virial mass. The three lines in each plot represent different choices of Λm^{3}. The blue solid line has Λm^{3} = 0.1 × 10^{3} eV^{4}/c^{8}, the dotted red line has Λm^{3} = 0.2 × 10^{3} eV^{4}/c^{8}, and the dashed black line has Λm^{3} = 0.3 × 10^{3} eV^{4}/c^{8}. 
2.6. Determining the virial radius
In the previous section we began by defining a central potential Φ_{0} and from this we determined the core radius as well as the core density. We therefore have at our disposal all the necessary components to determine the density of the DM fluid both inside and outside the core.
The next stage is to determine the radius at which to truncate the DM halo. In the ΛCDM paradigm, this is commonly defined for clusters as r_{200}, the radius at which the average density falls to 200 times the critical density of the Universe at a given redshift (Vikhlinin et al. 2006), that is, the virial density. We adopt this convention in our model. The mass M(R_{vir}) is then determined by evaluating Eq. (14) such that the above convention is respected at R_{vir}.
2.7. Making mass the free parameter
We have now determined a simplified way to model a spherical system in the superfluid framework. However, this was achieved by initially solving Poisson’s equation, which in turn required the input of the central potential Φ_{0} as a free parameter. A more ideal setup would be to determine all relevant quantities, R_{c}, ρ_{c}, R_{vir}, and Φ_{0} from a known total mass M_{vir}. This is possible with the aid of interpolation. The above procedure for a discrete set of n initial central potential values might be carried out, for example, { Φ_{01},Φ_{02},...,Φ_{0n} }. From this set an array of core radii is built, { R_{c01},R_{c02},...,R_{c0n} }, as well as core densities { ρ_{c01},ρ_{c02},...,ρ_{c0n} }, virial radii { R_{vir01},R_{vir02},...,R_{vir0n} } , and virial masses { M_{vir01},M_{vir02},...,M_{vir0n} }. Plots of Φ_{0} vs. M_{vir}, R_{c} vs. M_{vir}, ρ_{c} vs. M_{vir}, and R_{vir} vs. M_{vir} are then possible. Then, interpolation procedures can be implemented to make continuous functions of virial mass as functions of core radius, core density, central potential, and virial radius. This allows picking a virial mass and easily determining the required parameters that describe the fluid.
3. A worked example without baryons
We first illustrate here our procedure for a DMonly galaxy cluster, that is, without baryons, and with an isothermal normal phase. Figure 1 shows the interpolation functions for the core radius R_{c}, density at core radius ρ_{c}, central potential Φ_{0}, and superfluid core mass M_{c} as functions of the virial mass M_{vir}, following the procedure outlined in Sect. 2.7. These allow us to determine the correct parameters for a given total virial mass. In this example we chose a total mass of 10^{15}M_{⊙} at redshift z = 0.
Figure 1 shows that R_{c}, ρ_{c} and Φ_{0} all scale with virial mass by powerlaw profiles. We can try to understand this by analysing the model at the core radius. Firstly, ignoring baryons, Eq. (15) can by simplified to (17)To understand the origin of the power laws, we did not perform a rigorous calculation, but instead used approximations and dimensional analysis to reason that the numerical results are reasonable. As mass is proportional to volume and density, we can make the approximate proportional relation, . Therefore Eq. (17) can be interpreted as . We can also make the approximation that the velocity v is proportional to the virial velocity v_{vir}, which in turn we assume is proportional to the sound speed c_{s}. From our knowledge of the sound speed from Sect. 2.2 we know that . From our Poisson equation we also know . Therefore v_{vir} ∝ ρ_{c}. The virial radius is related to the virial mass as . Thus from the relation for circular velocity, we obtain . Collecting all these approximations, we obtain the following scaling relations:
which are in agreement with our numerical results. Although very informal, this analysis allows us to make an educated guess as to how the quantities might scale with each other. These scaling relations will not hold in the case when baryons are included, however.
We also show in Fig. 2 how varying the Λm^{3} parameter affects the results. When we increase Λm^{3}, we find a smaller R_{c}, larger ρ_{c}, and lower M_{c}, at the same virial mass. On the other hand, Φ_{0} remains unchanged. Again, this dependence can be understood on dimensional grounds. Specifically, the Λm^{3} scaling relations are
These scaling relations can be understood by looking at the dimensionless form of Eqs. (8) and (15). Omitted here for conciseness, it can be shown that a dimensionless core radius parameter arises from the Poisson equation, (20)This can also be understood from straightforward dimensional analysis; note that K has the dimension of density per velocity. The same x_{c} arises in the pressurebalancing condition (Eq. (15)), which then fixes x_{c} as a numerical constant for all halos. As x_{c} is constant, we gain information that scale as K^{2}.
Under the condition of a small core, that is, R_{c} ≪ R_{vir}, hence M_{c} ≪ M_{vir}, we obtain from Eq. (14) the relation (21)We therefore have two relations, which, together with , fix the scaling relations, ρ_{c} ~ Kv_{vir}, . The potential is independent of K. We can finally use Eq. (17) to find the M_{c} dependence.
These are in good agreement with the numerical results. To highlight this, in Fig. 2 we plot the dependence of R_{c}, ρ_{c}, and M_{c} on Λm^{3} for a fixed virial mass. We do not include the plot of Φ_{0} as it is not affected by changing Λm^{3}, which we checked numerically. Figure 2 follows the relationships shown in Eq. (19).
Fig. 2 Change in core radius (top panel), density at core radius (middle panel), and core mass (bottom panel) as a result of different values of Λm^{3}. This is a visual representation of the relationships listed in Eq. (19). 
As we have the relationship of the superfluid parameters with the virial mass and Λm^{3}, we can determine the correctly normalised scaling relations for the core radius, density at core radius, central potential, and the core mass. These are
These only rigorously apply for the situation where the baryon contribution is omitted and the normal phase is isothermal.
Figure 3 shows the range of DM density profiles in our model for different parameter choices (blue shaded region), together with an NFW profile of concentration c_{200} = 4 (black dashed line) for comparison. The virial mass is the same in the two cases, M_{vir} = 10^{15}M_{⊙}. The blue dots highlight the core radius for different choices of Λm^{3}. We see that the superfluid density is relatively constant within the core, as expected. Outside the core, the density profile transitions to the normalphase, isothermal profile with ρ ~ 1 /r^{2}. We can see from Fig. 3 that the core radius we calculate is approximately 50−100 kpc for different parameter choices.
Fig. 3 DM only density profile for our SfDM toy model with Λm^{3} = 0.1−0.3 × 10^{3} eV^{4}/c^{8} (blue shaded) and a c_{200} = 4ΛCDM NFW comparison profile (dashed black line) each with a virial mass of 10^{15}M_{⊙}. Blue circles show the radii of the superfluid core for different Λm^{3} choices (the upper line represents a larger choice of Λm^{3}, which results in a higher density and smaller core radius). Inside the core, the density is approximately constant, outside the core the density follows a strict isothermal 1 /r^{2} power law. The inclusion of baryons in this model will not affect the general features too much, but will shrink the core radius slightly. The core radius can be increased by using a smaller value of Λm^{3}, which we show in the following sections of the paper. 
We truncated the density to zero at the virial radius. If left untruncated, the enclosed mass would keep growing linearly, which is unphysical. Although the choice of the virial radius is somewhat arbitrary, as mentioned earlier, we chose r_{200} because this is commonly adopted in the literature.
To highlight the continuity of density and pressure, we show in Fig. 4 pressure vs. density (top panel) and sound speed vs. radius (bottom panel). Both the pressure and density are continuous, and thus we have satisfied our phasematching criteria. However, we note a sudden jump in gradient at the core radius. This is due to our requirement that density and pressure must be continuous, but not a continuity of the equation of state. This results in a discontinuous sound speed. This is perhaps a limitation of our model and our simplified transition between the superfluid and normal phase of DM. We do not address this matter here.
Fig. 4 Top panel: pressure vs. density for a DMonly model. Both the pressure and density are continuous, as per our phase transition requirements. At the core radius (black circle), the gradient jumps because of the discontinuity in the equation of state at the transition between the superfluid and normal phase of DM. The core radius is located very close to the rightmost part of the plot as the density is approximately constant within the core. Bottom panel: sound speed of DM (). The jump at the core radius (vertical line) results from the discontinuous equation of state at the boundary. This might be a consequence of our simplified model of the phase transition. Addressing this issue is best left for future work. Both panels have Λm^{3} = 0.3 × 10^{3} eV^{4}/c^{8}. 
We previously mentioned that in reality, the superfluid core would continue radially until its density dropped to zero. There should be a transition zone within which the superfluid and normal phases coexist. Introducing this feature would make the model much more complex, as understanding how to define the normalphase profile would become more challenging.
Simplicity is the actual reason for adopting our twophase model with the core radius occurring when the density and tangential pressure are continuous. The result of this is a superfluid phase that has a much smaller radial extent than the true model, meaning that the core radii values we quote here are underestimated.
To highlight this, we plot the superfluidonly density profile for a DMonly model (Fig. 5) without considering the normal phase. The “true” core radius is the point where ρ_{s} = 0. However, the normal phase should already be dominating at this stage. There is thus a whole “transition zone” in which the relative contribution of the normal phase would rise while the superfluid density sharply decreases.
We indicate the core radius we adopt for this work in the plot (black circle for an NFWlike normal phase and a black square for an isothermal normal phase). The “true” core radius at which ρ_{s} = 0 is approximately twice the value we determine from our pressurematching method for the isothermal case and approximately three times the value we determine for our NFW case.
We can therefore conclude that we expect, in reality, superfluid phonon behaviour to occur at larger radii than we present here. Although the NFW case predicts the density and pressure to match at a smaller radius than the isothermal case, the “true” physical core radius would be unaffected. For a future more realistic model, we need to investigate to which degree introducing a mixing phase would affect the galaxy clusters. This is beyond the scope of the present exploratory work.
Fig. 5 Superfluidonly density profile for aDMonly system with central gravitational potential Φ_{0} = −10^{12} m^{2} s^{2} and Λm^{3} = 0.3 × 10^{3} eV^{4}/c^{8}.The “true” core radius at which the effect of phonons disappears completely is where the superfluid density drops to zero. However, in the modelling presented in this paper, DM is considered to be entirely in the normalphase (nonsuperfluid) beyond the radius at which the tangential pressure is matched (what we call R_{c}). This matching radius is illustrated by a square for the isothermal case, and a circle shows the NFW normalphase case. We show this to emphasise that our method truncates any superfluid phonon effects at a smaller radius than the true radius of the superfluid matter. This is a feature of our simplified model, and more complex models will have to be constructed in the future to fully understand the superfluid paradigm. 
4. Application to galaxy cluster mass profiles
After outlining the procedure for calculating the DM density profile, we turn to a sample of galaxy clusters to check whether the superfluid paradigm provides a good description of the dynamical mass deduced from the temperature profile of Xray emitting gas in clusters, assuming hydrostatic equilibrium.
To determine how well the superfluid paradigm describes real galaxy clusters, we therefore compare the expected DM profile, determined from our aforementioned simplified superfluid modelling, to the actual mass of galaxy clusters deduced from the temperature profile of the Xray emitting gas. This amounts to a comparison of the enclosed mass derived from integrating the density profile of our model and the mass derived from hydrostatic equilibrium arguments. We have discussed how the enclosed mass derived from the density profile would be calculated (see Eq. (14)). We now briefly discuss how we derived the dynamical mass, that is, the mass derived from the Xray gas emission profile.
Our treatment makes a number of simplifying assumptions that are common when modelling the mass profile of galaxy clusters. Firstly, the gas in the cluster is treated as an ideal gas, and secondly, the cluster is assumed to be in hydrostatic equilibrium. By assuming this, the following equation can be constructed linking the dynamical (or total) mass M_{dyn}(r) of the system within a radius r, (26)Here, ρ_{g} is the gas density, P_{g} its pressure (linked to density and temperature through the ideal gas equation of state), and M_{dyn}(r) is the dynamical mass.
The dynamical mass is defined as the required amount of mass such that the gas temperature profile in hydrostatic equilibrium can be explained by Newtonian gravity. This mass can be compared to M_{grav} from Eq. (14). In ΛCDM and our superfluid cluster model the gravitational mass should be equivalent to the baryons + DM. In MOND the gravitational mass would be baryons + phantom dark matter. A phantom component in the superfluid paradigm arises from the phonons, which should be negligible in clusters.
We have selected a sample of four galaxy clusters from Vikhlinin et al. (2006). At this stage, we only tested the model on a few clusters to gain an understanding of the current model predictions. We expect similar results for the other clusters in the Vikhlinin et al. (2006) sample and therefore consider it sufficient to leave extending the sample size for future work when the model is developed further. In this work, analytic profiles were prescribed for both the gas density and temperature. Fitting routines were then run to determine the parameters for each model. This allows the dynamical mass to be calculated analytically. Firstly, the gas emission profile and temperature profile are defined in Eqs. (3) and (6) of Vikhlinin et al. (2006), respectively. The emission profile described in Vikhlinin et al. (2006) is essentially a superposition of two β density profiles that are commonly used when describing galaxy gas density. Vikhlinin et al. (2006) added in the extra components to account for the steepening brightness at r ≈ 0.3r_{200} and to impose a cuspy core to better match observations. More explicit details of this profile can be found in Vikhlinin et al. (2006).
In addition to the gas component, we also need to take the brightest cluster galaxy (BCG) into account, which is the large central galaxy component of the cluster. We modelled the baryonic component of the BCG using a Hernquist profile (Hernquist 1990), (27)where M is the mass of the BCG and h is the BCG scale radius. The Hernquist profile is an appropriate choice for modelling the BCG baryonic mass content as it provides a constantmass profile at large radii, resulting in a welldefined size or radius of the BCG. We adopted the BCG mass from Schmidt & Allen (2007), where the baryonic mass is approximated 1.14 × 10^{12}M_{⊙} for each cluster. In their model, they used a Jaffe profile with a scale length of ≈30 kpc. The Jaffe model has a slightly steeper density profile in the centre than the Hernquist model, which we mimicked by using a Hernquist scale radius of 10 kpc. Therefore the baryonic mass that we used when deriving the DM profile is the sum of the BCG and the gas masses. This is a crude approximation, and further work into understanding how large a BCG is required to fit the data is required. We note that there does not seem to be a consistent way to prescribe the BCG mass in galaxy clusters. Current techniques include assuming a constant masstolight ratio (e.g. Angus et al. 2008) or imposing a dependence on the total mass (e.g. Chiu et al. 2016). The reason this is not explored here is that the data in the centre of the cluster (30 kpc) are quite poor. A better study might be to use a galaxy cluster sample with stronglensing data such as Umetsu et al. (2016) to model the BCG more accurately. The accuracy of the central data might be increased as the assumption of hydrostatic equilibrium is not required for lensing.
The derived mass profiles are plotted in Fig. 6 for the isothermal normal phase and in Fig. 7 for the NFW normal phase.
Fig. 6 Enclosed mass profiles for the cluster sample. Red shaded regions show the ± 20% values of the dynamical mass calculated via Eq. (26). The blue shaded region shows the mass profile of the SfDM paradigm to highlight the Λm^{3} dependence (upper and lower bands represent a larger and smaller choice of Λm^{3}, respectively). We chose parameters Λm^{3} = (0.1−0.3) × 10^{3} eV^{4}/c^{8}. The black dashed line represents the NFW profile as given in Vikhlinin et al. (2006). Blue circles show the superfluid core radii for the upper and lower choices of Λm^{3}. The bestfit analytical gas and temperature profiles did not force monotonically increasing dynamical masses. To account for this, we removed unphysical features from the plot. Top left: A133 with a virial mass of 6 × 10^{14}M_{⊙}, top right: A262 with a virial mass of 2 × 10^{14}M_{⊙}, bottom left: A478 with a virial mass of 1.5 × 10^{15}M_{⊙}, and bottom right: A1413 with a virial mass of 1.5 × 10^{15}M_{⊙}. 
Fig. 7 Same as Fig. 6 for the NFW normal phase. Only the case of Λm^{3} = 0.3 × 10^{3} eV^{4}/c^{8} is shown. r_{s} for each cluster is defined as a fraction 1 /n of the virial radius, where n is 5, 6, 4, and 4 for clusters A133, A262, A468, and A1413, respectively. The NFW normal phase follows the ΛCDM prediction much more closely than the isothermal normalphase model. Central regions are still consistently smaller than in the ΛCDM predictions, which needs to be investigated in further work. 
In these plots, we compare the superfluid mass (blue shaded region for Fig. 6 and blue line for Fig. 7) to the dynamical mass (red shaded region). We also show the bestfit NFW DM profile (black dashed line) as given in Vikhlinin et al. (2006) to compare the ΛCDM result to the superfluid result. In practice, the best Λ and m parameters should be determined for the theory, but this needs to be done in accordance with galaxy rotation curves. This is not attempted in this work.
4.1. Isothermal analysis
We first discuss the case where an isothermal normal phase is imposed. Figure 6 shows that our density matching is approximately in the range of 50−100 kpc for the clusters, depending on our choice of Λm^{3}. Beyond this, in our normal phase, the mass profile is not perfectly in conjunction with the data, which is mainly due to the simplicity of the isothermal profile. Moreover, we have assumed that no normal phase matter is present below our pressurematching radius. We imposed this because of modelling constraints at this stage, but future work should be conducted into how representative this assumption is compared to simulation of a cluster. Khoury and collaborators are currently working on this problem. Finally, although small, the phonon force might increase the mass budget slightly. Quantifying this is the next challenge. In short, with the limitations of the model in mind, the main mismatch between data and theory is the constantdensity core. In addition, the outer parts of the clusters should be better described by an NFW profile, as in the next subsection.
4.2. NFW normal phase
Owing to the simplicity of the isothermal model, other normalphase profiles need to be tested. A natural choice is one that mimics the behaviour of the NFW profile (see Eq. (13)). We show the results for this in Fig. 7. For this figure, we only show the results for the higher value of Λm^{3} from our isothermal analysis. We can immediately see two consequences of imposing this normalphase component. Firstly, the outer profile is more in accordance with the data than the isothermal profile, as expected. The second consequence is that as expected from Fig. 5, the pressure matching occurs at a smaller radius. Therefore, for the same choice of Λm^{3} parameter, the NFW normal phase halo can match the data for a wider range of radii than for the isothermal case. We must again stress that the physical size of the “true” superfluid core (where the superfluid density drops to zero) would be the same in both cases.
4.3. Discrepancy in the centre
In ΛCDM, as mentioned, the commonly used DM profile is the NFW model, which is cuspy in the centre. Because a superfluid phase is included, the DM in our model has a cored profile. Therefore, to be consistent, the cuspyness in our model is achieved by the stellar BCG component. The BCG mass is not a wellconstrained property, hence the approximate model we use. We can conclude, however, that if the BCG mass is much lower in the central regions than we have estimated, a challenge to the superfluid description may arise. It is clear from Fig. 7 that the constantdensity superfluid core results in a systematic feature, the superfluid mass is lower than that predicted by ΛCDM. This could be rectified by using a slightly larger BCG, but this would need to be justified observationally. We also need to determine whether this systematic feature could be permitted within typical galaxy cluster mass error bars.
5. Discussion and conclusion
We have outlined a procedure for calculating spherical cluster models, embedded in a DM halo consisting of a superfluid. The simplified model assumes that DM exists in two distinct phases: a superfluid core, and a normalphase halo. We did not take into consideration a possible transition region with a mixture of superfluid and normalphase DM. This is left for further work. We tested two types of normal components: an isothermal profile, and NFWlike profile. The NFW was shown to produce better fits than the isothermal profile, although both models show a tendency to underpredict the mass in the centre in some cases because of the constant DM density core inherent to our present modelling. We stress that we also assumed that the phonon contribution to the force is negligible. This is a valid approximation as the phonon contribution adds a MONDlike force, which is known to be comparatively weak in clusters. This is certainly not valid in galaxies. However, the phonon contribution to the mass profile in the centre could play a role.
We applied our model to a set of galaxy clusters, comparing the mass derived from hydrostatic equilibrium and that of our superfluid model. We did not attempt to make a rigorous error analysis and χ^{2} fitting of the superfluid mass and the parameters that describe the superfluid, however. This needs to be done in conjunction with galaxies. Modelling galaxies is a much more complicated procedure because it must understood how the phonon contribution is to be modelled, and the spherical symmetry assumptions may need to be relaxed in order to correctly model disks. It is for these reasons that galaxies should be left for further analysis (Berezhiani et al., in prep.).We can conclude from the present analysis, however, that when a much lower value of Λm^{3} is needed in galaxies, the constantdensity core is extended in clusters, and this increase the discrepancy with data.
There is indeed some discrepancy between the superfluid result and the dynamical mass estimates of the cluster. For lower values of Λm^{3}, the superfluid core seems to systematically underpredict the mass profile in the galaxy cluster centre. This is a result of the superfluid recipe predicting a constantdensity core, whereas the data seem to prefer a cuspier central profile. This needs to be rigorously tested against stronglensing data of galaxy clusters as an independent test. We did achieve better fits with a larger choice of Λm^{3} at the cost of a smaller core radius, which could be in contention with galaxy data. However, as we mentioned, the true extent of the superfluid core will be larger than our quoted values, so this may not be an issue, and adding a phonon contribution to the centre might slightly alleviate the discrepancy.
The next goal is to perform lensing tests with galaxy clusters in the superfluid paradigm as an independent test. When this is completed, we may move on to model galaxies, with an understanding of how the phonon force can be included. In order to do this, we need to construct a more complicated model that includes a transition region between the superfluid and normal phase. With all these caveats in mind, the present work nevertheless gives an orderofmagnitude estimate of the parameter values of the theory that do not violently disagree with cluster data. If much lower values of Λm^{3} were needed in galaxies, it would be difficult to reconcile the superfluid DM framework with galaxy clusters.
Acknowledgments
We thank Lasha Berezhiani for helpful discussions. We also thank Alexey Vikhlinin for helpful correspondence on the cluster data. We warmly thank Priya Natarajan and Doug Finkbeiner for hosting a stimulating Radcliffe Exploratory Seminar at Harvard University where this collaboration was initiated. We would also like to thank the anonymous referee for their helpful comments on style and content that improved the paper. A.O.H. is supported by Science and Technologies Funding Council (STFC) studentship (Grant code: 1APAASTFC12). J.K. is supported in part by NSF CAREER Award PHY1145525, NASA ATP grant NNX11AI95G, and the Charles E. Kaufman Foundation of the Pittsburgh Foundation. B.F. acknowledges financial support from the “Programme Investissements d’Avenir” (PIA) of the IdEx from the Université de Strasbourg.
References
 Angus, G. W. 2009, MNRAS, 394, 527 [NASA ADS] [CrossRef] [Google Scholar]
 Angus, G. W., Famaey, B., & Buote, D. A. 2008, MNRAS, 387, 1470 [NASA ADS] [CrossRef] [Google Scholar]
 Bekenstein, J., & Milgrom, M. 1984, ApJ, 286, 7 [NASA ADS] [CrossRef] [Google Scholar]
 Berezhiani, L., & Khoury, J. 2015, Phys. Rev. D, 92, 103510 [NASA ADS] [CrossRef] [Google Scholar]
 Berezhiani, L., & Khoury, J. 2016, Phys. Lett. B, 753, 639 [NASA ADS] [CrossRef] [Google Scholar]
 Blanchet, L., & Heisenberg, L. 2015, Phys. Rev. D, 91, 103518 [NASA ADS] [CrossRef] [Google Scholar]
 BoylanKolchin, M., Bullock, J. S., & Kaplinghat, M. 2011, MNRAS, 415, L40 [CrossRef] [Google Scholar]
 BoylanKolchin, M., Bullock, J. S., & Kaplinghat, M. 2012, MNRAS, 422, 1203 [NASA ADS] [CrossRef] [Google Scholar]
 Chiu, I., Mohr, J., McDonald, M., et al. 2016, MNRAS, 455, 258 [NASA ADS] [CrossRef] [Google Scholar]
 Clowe, D., Bradač, M., Gonzalez, A. H., et al. 2006, ApJ, 648, L109 [NASA ADS] [CrossRef] [Google Scholar]
 de Blok, W. J. G. 2010, Adv. Astron., 2010, 789293 [NASA ADS] [CrossRef] [Google Scholar]
 Desmond, H. 2017, MNRAS, 464, 4160 [CrossRef] [Google Scholar]
 Di Cintio, A., & Lelli, F. 2016, MNRAS, 456, L127 [NASA ADS] [CrossRef] [Google Scholar]
 Dubinski, J., & Carlberg, R. G. 1991, ApJ, 378, 496 [Google Scholar]
 Famaey, B., & McGaugh, S. S. 2012, Liv. Rev. Rel., 15, 10 [Google Scholar]
 Hernquist, L. 1990, ApJ, 356, 359 [Google Scholar]
 Hodson, A., & Zhao, H. 2017a, A&A, 598, A127 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
 Hodson, A. O., & Zhao, H. 2017b, A&A, 608, A109 [CrossRef] [EDP Sciences] [Google Scholar]
 Hui, L., Ostriker, J. P., Tremaine, S., & Witten, E. 2017, Phys. Rev. D, 95, 043541 [NASA ADS] [CrossRef] [PubMed] [Google Scholar]
 Ibata, R. A., Lewis, G. F., Conn, A. R., et al. 2013, Nature, 493, 62 [CrossRef] [Google Scholar]
 Keller, B. W., & Wadsley, J. W. 2017, ApJ, 835, L17 [NASA ADS] [CrossRef] [Google Scholar]
 Khoury, J. 2015, Phys. Rev. D, 91, 024022 [NASA ADS] [CrossRef] [Google Scholar]
 Khoury, J. 2016, Phys. Rev. D, 93, 103533 [NASA ADS] [CrossRef] [Google Scholar]
 Klypin, A., Kravtsov, A. V., Valenzuela, O., & Prada, F. 1999, ApJ, 522, 82 [Google Scholar]
 Lee, J.W. 2016, Phys. Lett. B, 756, 166 [NASA ADS] [CrossRef] [Google Scholar]
 Lelli, F., McGaugh, S. S., & Schombert, J. M. 2016, ApJ, 816, L14 [Google Scholar]
 Ludlow, A. D., BenítezLlambay, A., Schaller, M., et al. 2017, Phys. Rev. Lett., 118, 161103 [NASA ADS] [CrossRef] [Google Scholar]
 McGaugh, S., Lelli, F., & Schombert, J. 2016, Phys. Rev. Lett., 117, 201101 [NASA ADS] [CrossRef] [Google Scholar]
 Milgrom, M. 1983a, ApJ, 270, 371 [Google Scholar]
 Milgrom, M. 1983b, ApJ, 270, 384 [NASA ADS] [CrossRef] [Google Scholar]
 Milgrom, M. 1983c, ApJ, 270, 365 [NASA ADS] [CrossRef] [Google Scholar]
 Moore, B., Ghigna, S., Governato, F., et al. 1999, ApJ, 524, L19 [Google Scholar]
 Navarro, J. F., Frenk, C. S., & White, S. D. M. 1997, ApJ, 490, 493 [NASA ADS] [CrossRef] [Google Scholar]
 Navarro, J. F., BenítezLlambay, A., Fattahi, A., et al. 2017, MNRAS, 471, 1841 [NASA ADS] [CrossRef] [Google Scholar]
 Oman, K. A., Navarro, J. F., Fattahi, A., et al. 2015, MNRAS, 452, 3650 [CrossRef] [Google Scholar]
 Pawlowski, M. S., Famaey, B., Merritt, D., & Kroupa, P. 2015, ApJ, 815, 19 [NASA ADS] [CrossRef] [Google Scholar]
 Sanders, R. H. 1999, ApJ, 512, L23 [NASA ADS] [CrossRef] [Google Scholar]
 Sanders, R. H. 2003, MNRAS, 342, 901 [NASA ADS] [CrossRef] [Google Scholar]
 Schmidt, R. W., & Allen, S. W. 2007, MNRAS, 379, 209 [NASA ADS] [CrossRef] [Google Scholar]
 Umetsu, K., Zitrin, A., Gruen, D., et al. 2016, ApJ, 821, 116 [Google Scholar]
 Vikhlinin, A., Kravtsov, A., Forman, W., et al. 2006, ApJ, 640, 691 [NASA ADS] [CrossRef] [Google Scholar]
 Walker, M. G., & Peñarrubia, J. 2011, ApJ, 742, 20 [NASA ADS] [CrossRef] [Google Scholar]
 Zhao, H. 1996, MNRAS, 278, 488 [Google Scholar]
 Zhao, H., & Famaey, B. 2012, Phys. Rev. D, 86, 067301 [NASA ADS] [CrossRef] [EDP Sciences] [Google Scholar]
All Figures
Fig. 1 Toy model of a DMonly system. We highlight the dependence of the superfluid parameters on the choice of virial mass for a system that only includes DM. We stress that this result does not consider baryons, and a more complete analysis should be performed, which we provide for the cluster sample. If we were to include baryons, we would expect to see a slight decrease in core radius for our clusters. This difference would be enhanced in galaxies. Top left: core radius vs. virial mass. Top right: density at the core radius vs. virial mass. Bottom left: central potential vs. virial mass. Bottom right: superfluid core mass vs. virial mass. The three lines in each plot represent different choices of Λm^{3}. The blue solid line has Λm^{3} = 0.1 × 10^{3} eV^{4}/c^{8}, the dotted red line has Λm^{3} = 0.2 × 10^{3} eV^{4}/c^{8}, and the dashed black line has Λm^{3} = 0.3 × 10^{3} eV^{4}/c^{8}. 

In the text 
Fig. 2 Change in core radius (top panel), density at core radius (middle panel), and core mass (bottom panel) as a result of different values of Λm^{3}. This is a visual representation of the relationships listed in Eq. (19). 

In the text 
Fig. 3 DM only density profile for our SfDM toy model with Λm^{3} = 0.1−0.3 × 10^{3} eV^{4}/c^{8} (blue shaded) and a c_{200} = 4ΛCDM NFW comparison profile (dashed black line) each with a virial mass of 10^{15}M_{⊙}. Blue circles show the radii of the superfluid core for different Λm^{3} choices (the upper line represents a larger choice of Λm^{3}, which results in a higher density and smaller core radius). Inside the core, the density is approximately constant, outside the core the density follows a strict isothermal 1 /r^{2} power law. The inclusion of baryons in this model will not affect the general features too much, but will shrink the core radius slightly. The core radius can be increased by using a smaller value of Λm^{3}, which we show in the following sections of the paper. 

In the text 
Fig. 4 Top panel: pressure vs. density for a DMonly model. Both the pressure and density are continuous, as per our phase transition requirements. At the core radius (black circle), the gradient jumps because of the discontinuity in the equation of state at the transition between the superfluid and normal phase of DM. The core radius is located very close to the rightmost part of the plot as the density is approximately constant within the core. Bottom panel: sound speed of DM (). The jump at the core radius (vertical line) results from the discontinuous equation of state at the boundary. This might be a consequence of our simplified model of the phase transition. Addressing this issue is best left for future work. Both panels have Λm^{3} = 0.3 × 10^{3} eV^{4}/c^{8}. 

In the text 
Fig. 5 Superfluidonly density profile for aDMonly system with central gravitational potential Φ_{0} = −10^{12} m^{2} s^{2} and Λm^{3} = 0.3 × 10^{3} eV^{4}/c^{8}.The “true” core radius at which the effect of phonons disappears completely is where the superfluid density drops to zero. However, in the modelling presented in this paper, DM is considered to be entirely in the normalphase (nonsuperfluid) beyond the radius at which the tangential pressure is matched (what we call R_{c}). This matching radius is illustrated by a square for the isothermal case, and a circle shows the NFW normalphase case. We show this to emphasise that our method truncates any superfluid phonon effects at a smaller radius than the true radius of the superfluid matter. This is a feature of our simplified model, and more complex models will have to be constructed in the future to fully understand the superfluid paradigm. 

In the text 
Fig. 6 Enclosed mass profiles for the cluster sample. Red shaded regions show the ± 20% values of the dynamical mass calculated via Eq. (26). The blue shaded region shows the mass profile of the SfDM paradigm to highlight the Λm^{3} dependence (upper and lower bands represent a larger and smaller choice of Λm^{3}, respectively). We chose parameters Λm^{3} = (0.1−0.3) × 10^{3} eV^{4}/c^{8}. The black dashed line represents the NFW profile as given in Vikhlinin et al. (2006). Blue circles show the superfluid core radii for the upper and lower choices of Λm^{3}. The bestfit analytical gas and temperature profiles did not force monotonically increasing dynamical masses. To account for this, we removed unphysical features from the plot. Top left: A133 with a virial mass of 6 × 10^{14}M_{⊙}, top right: A262 with a virial mass of 2 × 10^{14}M_{⊙}, bottom left: A478 with a virial mass of 1.5 × 10^{15}M_{⊙}, and bottom right: A1413 with a virial mass of 1.5 × 10^{15}M_{⊙}. 

In the text 
Fig. 7 Same as Fig. 6 for the NFW normal phase. Only the case of Λm^{3} = 0.3 × 10^{3} eV^{4}/c^{8} is shown. r_{s} for each cluster is defined as a fraction 1 /n of the virial radius, where n is 5, 6, 4, and 4 for clusters A133, A262, A468, and A1413, respectively. The NFW normal phase follows the ΛCDM prediction much more closely than the isothermal normalphase model. Central regions are still consistently smaller than in the ΛCDM predictions, which needs to be investigated in further work. 

In the text 
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