# Environmental Mechanisms Shaping the Nature of Dwarf Spheroidal Galaxies: The View of Computer Simulations

Authors: Lucio Mayer
Journal: Advances in Astronomy
 (2010)

---

## Abstract

We review numerical works carried out over the last decade on the role of environmental mechanisms in shaping nature of the faintest galaxies known, dwarf spheroidals (dSphs).
The combination of tidally induced morphological
transformation, termed tidal stirring, with mass loss due to tidal and ram-pressure stripping aided by heating due to the cosmic ionizing background can turn late-type dwarfs resembling present-day dIrrs into classic dSphs.
The time of infall into the primary halo is shown to be a key parameter. Dwarfs accreting atz>1, when the
cosmic ultraviolet ionizing flux was much higher than today, and was thus able to keep the gas in the dwarfs warm and diffuse, were rapidly stripped of their baryons via ram pressure and tidal forces, producing very dark-matter-dominated objects with truncated star-formation histories, such as the Draco dSph. The low star-formation efficiency expected in such low-metallicity objects prior to their infall was crucial for keeping their disks gas dominated until stripping took over. Therefore gas stripping along with inefficient star-formation provides a new feedback mechanism, alternative to photoevaporation or supernovae feedback, playing a crucial role in dwarf galaxy formation and evolution. We also discuss how the ultra-faint dSphs belong to a different population of lower-mass dwarf satellites that were mostly shaped by reionization rather than by environmental mechanisms (“reionization fossils”). Finally, we scrutinize the various caveats in the current understanding of environmental effects as well as other recent ideas on the origin of Local Group dSphs.


---

## Body

## 1. Introduction

Dwarf spheroidals (dSphs) in the Local Group are the faintest galaxies known. Including the ultrafaint dwarf spheroidals discovered in the last few years, they span luminosities in the range-3<MB<-14. They are gas poor and have pressure supported stellar components [1]. Among them, some stopped forming stars about 10 Gyr ago and others have extended star-formation histories [2–4]. They are typically clustered around the largest galaxy in a group, although a few of them are found also at significantly larger distances from the primary galaxy [1]. These properties of dSphs, while best studied and known in the Local Group due to its proximity, are also typical of this class of galaxies in nearby groups and clusters. Chiboucas, Karachentsev, and Tully [5] have recently uncovered a population of dSphs in the M81 group having a range of luminosities comparable to the LG dwarfs and which share with the latter the same scaling relations between fundamental structural properties, such as the relation between luminosity and effective radius. Recent studies of early-type dwarfs in clusters [6] show that there is overlap in the structural properties between the faint spheroidals in clusters and the classic dSphs in the LG, as shown by the size-luminosity and the surface brightness-luminosity relations. Strong similarities between dSphs in the LG and in clusters are also found by Penny et al. [7] in their study of the Perseus cluster. Hence, LG dSphs can be considered a representative laboratory for the study of dSphs in the Universe. Mass loss from supernovae winds [8], environmental mechanisms such as tidal and ram pressure strippings [9, 10] and suppression, of gas accretion and/or photoevaporation during the reionization epoch [11, 12] have all been invoked to explain their origin and present-day properties. In this paper we review the current status of theoretical models attempting to explain dwarf spheroidals as the end product of environmentally induced morphological transformations from larger, gas-rich disky galaxies [13, 14]. The transformation scenario is suggested by the fact that gas-rich, disky dwarf irregular galaxies (dIrrs) and dSphs have similar stellar density profiles, close to exponential laws [10], and obey the morphology-density relation whereby dIrrs are found in the outskirts of groups while dSphs are mainly clustered around the main galaxy [1, 15]. In hierarchical structure formation, subhalos nearer to the center of a virialized group halo or galaxy-sized halo were accreted earlier [16]; they were once beyond the edge of the primary halo removed from its tidal influence. We discuss how the combination of tidal effects, ram pressure stripping and the cosmic ultraviolet background radiation at high redshift may provide an explanation to both the similarities and differences among the many known Local Group dwarf spheroidal galaxies. We place our analysis in the context of the current paradigm for structure formation, the ΛCDM model. In this review we will always distinguish between classic dSphs [1], those that were known even before the advent of the SDSS deep photometric survey and have luminosities MB<-7, and the ultrafaint dwarfs discovered by the SDSS, whose luminosities reach as low as MB~-3 (e.g., [17]). The classic dwarfs include Draco, Ursa Minor, Sculptor, Sextans, Leo I and Leo II, Carina, Sagittarius, Cetus, and Tucana among the companions of the Milky Way, and the many “And” satellites of M31. Based on the current measures of their internal stellar velocity dispersions and on theoretical predictions on tidal mass loss of subhalos, we will argue that classic dwarf spheroidals were assembled in fairly massive halos, with masses in the range 108-1010M⨀. For these dwarfs, reionization played some role in depleting their baryonic content enhancing the effect of gas removal mechanisms such as tidal stripping and tidal stirring as well as ram pressure stripping. Such mechanisms were the major drivers of their evolution. On the contrary, the low halo masses of ultrafaint dwarfs make them likely candidates for reionization fossils. The theoretical models that we present here are based on the results of N-Body+hydrodynamical simulations of the detailed interaction of individual dwarf galaxies with a primary host, as well as of high-resolution cosmological simulations of Milky-Way-sized galaxies.In the interaction simulations, the model galaxies and the choice of the orbits are consistent with the predictions of ΛCDM models [18–20].


## 2. Current and Past Masses of Dwarf Spheroidals: Why Tides Are Important

Knowing the present and past masses of dSphs is crucial in order to compute the effects of both environmental and internal mechanisms that might affect their evolution. Moreover, determining the mass of dSphs, or, equivalently, their circular velocity, plays a crucial role in the context of the missing satellites problem [21, 22]. Here we will concentrate on the effects that tides have on the evolution of the mass and circular velocity of subhalos of Milky-Way-sized halos, and we will discuss how this folds in with the interpretation of the mass and circular velocity measured for observed dwarf spheroidals.In cold dark matter models, subhalos are accreted on highly eccentric orbits, with a mean apocenter-to-pericenter ratio of 5-6 [16, 23–25]. Since the orbits are eccentric, subhalos feel a time-dependent tidal force whose intensity is strongest close to pericenter of their orbit. The system undergoes an increase of internal kinetic energy as a result of the tidal forcing, which modifies the energy and mass profile of the subhalo, eventually unbinding some of its stars or dark matter, namely producing tidal stripping. The system will then attempt to reach a new virial equilibrium with a lower gravitational binding energy, which in turn can make it more susceptible to the effect of subsequent tidal shocks as its internal orbital/dynamical time increases (see Binney & Tremaine 1987). If a new equilibrium cannot be achieved, the system will continue to expand, lower its gravitational binding energy, and lose mass, until it is eventually completely disrupted. At low eccentricities, the heating is reduced significantly, until it becomes completely absent for a strictly circular orbit [26].Tidal heating in an extended mass distribution is most effective when the internal dynamical time of the satellite is larger or at least commensurate with the characteristic timescale associated with the galaxy’s orbit [26–28]. In this case it can be described using an extension of the impulsive approximation valid for a generic elliptical orbit of the satellite [26], while the original impulsive approximation was derived for a pointlike perturber and a target (the satellite) moving on a straight-line path (Binney & Tremaine 1987). Following Gnedin et al. [26], the expression for the heating term per unit mass for an extended perturber, but approximating the orbit to a straight-line path, is 〈ΔE〉=(2GM0/VperiRperi2)(r2/3)χst(Rperi), where G is the gravitational constant, M0 is the mass of the perturber, Rperi and Vperi are, respectively, the pericenter distance and pericenter velocity, r is the distance of a member star from the center of the satellite, and χst is function that accounts for the form of the mass distribution of the perturber (it would be unity for a point mass). A more complex expression, but with similar scaling on the relevant variables, can be obtained for elliptical orbits. If, instead, the reverse condition applies to the two timescales, the system can readjust quickly to the perturbation and remain close to its original equilibrium configuration. This second situation can be described analytically by introducing the socalled adiabatic corrections. These are functions that reduce the mean relative increase of internal energy 〈ΔE〉/E derived via the impulsive approximation, their value being proportional to the internal orbital frequency of the system. Based on the same formalism, it is easy to see that the innermost region of any system, that has the highest density and thus the shortest dynamical time/orbital frequency, is also the one that responds more adiabatically to the tidal perturbation. The instantaneous orbital timescale, torb=2πRorb/Vorb, is shortest at pericenter of the orbit, that is, when Rorb=Rperi and Vorb=Vperi, which naturally implies that the effect of the tidal perturbation will be stronger there. Since the instantaneous orbital timescale, and thus the effect of the tidal perturbation, varies the most when the galaxy approaches or leaves pericenter, this is where the tidal force varies more strongly (recall that the tidal force is relatively short range, being proportional to r-3, where r is the distance from the center of the perturbing potential), hence the term “tidal shock”. If the orbit of the dwarf is circular, there is no tidal shock.Even before suffering the first tidal shock, a subhalo falling into the potential of the primary halo for the first time would lose mass located at a radiusr larger than its instantaneous tidal radius rt (the tidal radius of the subhalo decreases as it plunges closer to the center of the primary halo). This other stripping mode is often termed "tidal truncation". There are thus two mechanisms of tidal mass loss, tidal truncation, which typically shrinks the subhalo to a radius of order rt evaluated at the pericenter of its orbit, and tidal shocks [27, 29–31]. For subhalos with masses <1/50 of the mass of the primary halo, as true for most satellites of the Milky Way and M31 except perhaps the Large Magellanic Cloud, dynamical friction has a negligible effect [32], thereby one can assume that their orbits did not change since infall. The growth in mass and size of the primary halo over time also has been shown to have a negligible effect on the orbits of satellites in the case of a smoothly evolving analytical potential [33], although the clumpy and more erratic character of halo accretion and growth observed in cosmological simulations may still have an impact on orbital dynamics that should be investigated. With the assumption of a subhalo orbit constant over time, the tidal field of the primary near the pericenter of orbit is fixed over time. Tidal truncation thus occurs only on the first orbit. On the contrary, tidal shocks lead to continued mass loss on a fixed orbit since each subsequent shock can heat the satellite and alter progressively its internal structure. The process will cease to be effective only when the region heated by the shock is dense enough to respond adiabatically to the external perturbation or when the satellite is completely disrupted by tides. As shown in Figure 1, analytical models using a combination of tidal truncation on the first orbit and repeated tidal shocks describe well the mass loss seen in numerical simulations [27].Figure 1
Bound mass in units of the initial mass as a function of time, for a (dark-matter-only) satellite moving on an eccentric orbit within a Milky Way halo potential (see [27] for details). The mass of the satellite is 1/50 of the mass of the primary and both are modeled with NFW halos. The ratio between the concentration parameter of the halo and satellite is cs/ch=0.7, where ch=10 is the concentration of the primary halo. The symbols are the N-Body data and the solid line shows the results of the semianalytical model described in Taffoni et al. [27], that includes both tidal truncation and tidal shocks (see text). Stars identify each pericentre passage. The dashed line is the bound mass that would remain if only tidal truncation is applied.The amount of tidal mass loss of subhalos in numerical simulations can be remarkable. Kazantzidis et al. [34] have studied the disruption of CDM subhalos within a Milky-Way-sized primary with as many as 107 particles. This approach has the advantage of allowing much higher resolution in subhalos relative to a fully cosmological simulation that has to cope with modeling many objects simultaneously. Tidal mass loss was found to be more severe in less concentrated halos (where the concentration parameter is defined as the ratio c=rvir/rs, where rvir is the virial radius of the subhalo and rs is its scale radius, assuming an initial NFW profile) because they respond more impulsively owing to their lower characteristic density and, correspondingly, longer internal dynamical times. Subhalos typically lose between 70% and 95% of their mass depending on orbits and concentration. Correspondingly, their peak circular velocity, Vpeak, decreases by a factor 2-3 over ten billion years of tidal mass loss. Vpeak reflects the inner mass distribution of the subhalo, at radii of order rs, and is commonly used as a measure of the characteristic subhalo mass throughout literature. Its evolution over time is less strongly affected by tidal mass loss compared to the circular velocity of the subhalo at the virial radius. Subhalos initialized with cuspy NFW profiles maintain cuspy profiles with inner slopes close to -1 down to the force resolution, which in Kazantzidis et al. [34] was smaller than the core radius of dSphs (~100 pc) [35]. This result contradicts previous attempts to place dSphs within cored subhalos with the highest masses and Vpeak among the satellites' population in an attempt to solve the substructure problem [24, 36, 37].Kravtsov et al. [24], using fully cosmological dark matter-only simulations, found that Vpeak of the subhalos drops on average by a factor of 1.5–2 in 10 Gyr of tidal evolution. More recently, Diemand et al. [16] and Madau et al. [38], using the high-resolution Via Lactea simulation of the formation of a Milky-Way-sized halo, found that satellites lose between 30% and 99% of their preinfall mass and that Vpeak decreases typically by a factor of 2-3. This is consistent with the recent results of Klimentowski et al. [39, 40] on the mass loss of an ultra-high-resolution subhalo with embedded stellar disk (see Figure 3, top panel). Quantitatively similar results are obtained also in individual subhalo-primary interaction simulations in which gas dynamics with cooling and heating are included ([19, 20, 41], see also Section 5). Therefore there is now strong consensus on how tidal mass loss affects subhalos, both qualitatively and quantitatively.Peak velocities for the best fit models to observed dSphs are at most a factor of 2 higher than those used in Moore et al. [22] for subhalos, with the consequence that little changes for the missing satellite problem. Measurements of Vpeak, in both simulated subhalos and real satellite galaxies of the Local Group, are extremely important since they are used to express the missing satellite problem, namely, the excess in the number counts of subhalos at a given Vpeak compared to the counts of observed dSph satellites of the Milky Way and M31 ([21], Moore et al. 1998, [24]). However, in observed dSph satellites, one measures stellar velocity dispersions rather than the Vpeak of the subhalo. Going from stellar velocity dispersion to Vpeak requires assumptions when the only information available from simulations is that provided by the dark matter component. Typically (e.g., [34, 42]) one uses the radial moment of the Jeans equations to compute the relation between the circular velocity of the halo of the satellite and the velocity dispersion of the stars, using the simulated subhalo dark matter profile but adopting a simple functional form for a spherically symmetric stellar profile (typically a King model). In this approach it is also necessary to assume a value for the velocity anisotropy of the stellar system. As first shown by Lokas [42], anisotropy can play an important role in determining masses of dSphs from the data. By varying assumptions in the Jeans modeling, including anisotropy, S.Kazantzidis et al. [34] found that the observed stellar velocity dispersions of Draco and Fornax (σ~10–14 km/s) can be reproduced in subhalos with Vpeak~20–30 km/s. Similar results were obtained by Zentner and Bullock [43]. Finally, this range is confirmed also by a more recent analysis that adopts a similar methodology but takes advantage of the cosmological Via Lactea simulation [38, 44]. The latter work finds values closer to 15–20 km/s for some of the other dSphs (e.g., Carina and Sextans). In Madau et al. [38] a match between individual Local Group (LG) dwarf spheroidals and individual subhalos is achieved by considering information on the distances and spatial distribution of dwarfs. In any case, the values of Vpeak obtained by these recent works for dSphs are within a factor of 2 from those originally used in Klypin et al. [21] and Moore et al. [22] to formulate the substructure problem (note also that these two works did not use exactly the same conversion between circular velocity and stellar velocity dispersion, see Kravtsov in this volume).Recently, Klimentowski et al. [39, 40] have addressed the question of relating the observed line-of-sight stellar velocity dispersion σ1D of dSphs to the Vpeak of their halo using simulations that, albeit not fully cosmological, model both the baryonic and dark matter component of a disky dwarf subject to the tidal perturbation from a Milky-Way-sized galaxy (see below). They have found that the simple assumption that Vc~3σ1D, formally valid for a tracer stellar population in an isotropic dark matter halo and used by Klypin et al. [21], correctly describes the relation between the local stellar dispersion and the local halo circular velocity over a wide range of radii after 10 Gyr of evolution in the Milky Way potential (see Figure 3), as explained in the next section (intermediate phases in which the stellar velocity dispersion tensor is more anisotropic produce temporary deviations from this relation).In summary, the substantial simulation work carried out in the last few years suggests that stellar velocity dispersions of present-day classic dSphs of the MW and M31 in the rangeσ~7–13 km/s (7–20 km/s if we include the bright dwarf elliptical satellites of M31, NGC187, and NGC205) imply present-day halo Vpeak in the range 12–22 km/s, and original halo Vpeak, that is, before infall and tidal mass loss, in the range 24–44 km/s [24, 38]. These last numbers are quite important. In fact, with such relatively high values of the original Vpeak, photoevaporation by cosmic ultraviolet background at high redshift and supernovae feedback cannot be what shaped the baryonic content and nature of dwarf spheroidal as often advocated. In fact photoevaporation would remove most of the gas only for Vpeak<20 km/s [12]. This is consistent with the lack of a clear signature of the reionization epoch in the star-formation histories of dSphs [45, 46]. Second, substantial blowout of the gas of dSphs due to supernovae winds cannot have occurred since it requires Vpeak<10 km/s (e.g., [47, 48]). A caveat in the last line of reasoning is that in LCDM the progenitors of todays' dSphs formed by hierarchical accretion of smaller sublumps as any other galaxy and such sublumps might have had a mass low enough to be affected by both reionization and feedback. However, the old ages of the bulk of the stars in the majority of dwarf spheroidals mean that their star-formation epoch occurred more than 10 Gyr ago (z>2). While dating of stars is nonaccurate enough to establish how much of the old stellar component was formed before or after reionization, which occurred at z>6, the cosmic UV background was still close to its peak intensity at z=2 according to standard models [49,2000], and yet star formation was clearly happening. This argues against an important effect of the cosmic UV background arising from reioinization, perhaps owing to self-shielding (see [12]). Note that, conversely, there are examples of low mass LG dIrrs bearing a likely imprint of reionization in their star-formation history (e.g.; Leo A, see [50]).The same argument does not apply to the ultrafaint dwarf spheroidals discovered in the last few years using deep photometry from the Sloan Digital Sky Survey (SDSS) (e.g., [51, Belokurov et al. 2008,53]). With a few exceptions, most of the extremely faint dwarfs have very low velocity dispersions in the range 3–8 km/s [52], implying masses much lower than those of classic dSphs. We will discuss them in Section 8.For the classic dSphs, we advocated that physical processes associated with the environment, such as tidal forces and ram-pressure stripping, were the major players in setting their current properties and shaping their evolution. The remainder of this review will be devoted to summarizing in quite some detail the work done in this direction. In the next two sections, we will discuss how tidal interactions can completely reshape dwarf galaxies, presenting a plausible model for the origin of dwarf spheroidals in which such galaxies started out with a configuration and properties similar to gas-rich dwarf irregulars, and how these tidal interactions were subsequently transformed. We will also discuss the issue of measuring the masses of dwarf spheroidals from the observed stellar velocity dispersions, highlighting how tidal effects may produce contaminated samples with a fraction of unbound stars projected along the line of sight.


## 3. Morphological Evolution of Disky Dwarfs  into dSphs: Tidal Stirring

Aside from the different gas content, three other facts have to be considered when comparing dSphs and the other known type of dwarfs, namely, gas-rich, similarly faint dwarf irregular galaxies (dIrrs) (see [1] for a review on the subject). First, except for the faintest among them, all dIrrs in the Local Group and nearby groups exhibit substantial rotation while dSphs do not. Second, stellar profiles in the two classes of galaxies are similarly close to exponential. Third, a morphology density relation exists such that dSphs are clustered around the primary galaxies while dIrrs are found at much larger distances from them. Interestingly, Karachentsev [53] finds that the fraction of dSphs over the total number of dwarfs in several nearby groups (including the Local Group) decreases markedly at distances larger than about 250 kpc from the primary galaxies, comparable to the virial radius of halos hosting bright spiral galaxies in ΛCDM models. Clear trends of dwarf galaxy morphology with environment for nearby groups (Centaurus A and Sculptor) are also found by Bouchard et al. [54]. The quantitative correlation found by Karachentsev [53] strongly suggests, although it does not prove, that dSphs are bound satellites of bright spirals. It follows then automatically that the environment provided by the extended halo of such massive hosts must be playing a crucial role in differentiating dIrrs from dSphs. Of course there are outliers like the Local Group dSphs Cetus and Tucana, located at more than 500 kpc from, respectively, M31 and the MW. However, cosmological simulations provide a potential explanation for those few distant dSphs; a few satellite halos on very plunging orbits can have apocenters exceeding the virial radius of the primary [23], or can be on tighter orbits and subsequently be ejected out to much larger distances via three-body interactions (Sales et al. 2009). The outgoing radial velocity of Tucana further supports this possibility [55]. Overall, there are various effects that could make the orbital dynamics of satellites much more complex than in our simulation setup and accomodate such a case (see page 17-18).Mayer et al. [13, 14], Mayer [19], MA06, Mayer et al. [41], and Klimentowski et al. [39, 57] have shown that repeated tidal shocks at pericenters of their orbits within the halo of a massive spiral can transform infalling disky dwarfs into objects resembling dSphs. The timescale of the transformation is a few orbital times (several Gyr). The mechanism behind the transformation is tidally induced nonaxisymmetric instabilities of stellar disks combined with impulsive tidal heating of the stellar distribution. We recall that the time-dependent tidal field varies on a timescale proportional to the orbital timescale of the galaxy.The tidal forcing induces a perturbation to the internal energy and velocity distribution of the system, which results into a perturbation of its mass and density distribution as it attempts to acquire a new equilibrium configuration. Through the density perturbation tidal heating can thus excite modes in a self-gravitating system that would otherwise have a negligible amplitude. If the induced velocity and density perturbation are considerable, a strong mode might be seeded and be subsequently amplified by the self-gravity of the system. An example of such induced mode amplification is the triggering of a bar instability, which corresponds to anm=2 mode for the planar density field of the galaxy, of a warp, which corresponds to an m=1 in the vertical density field (i.e., perpendicular to the disk plane), or of a bending or buckling instability, which corresponds to an m=2 mode in the vertical density field [58]. Numerical experiments, starting from the early 90s, have shown that the buckling instability can be triggered by a preceding bar instability. A bar is supported by families of centrophilic stellar orbits, whose collective effect is to increase the radial velocity dispersion along the plane of the galaxy. Raha et al. [58] first showed that above some critical value of the radial velocity anisotropy, a system would become unstable to the buckling instability; the whole disk bends above and below, and, as a result, stars acquire a larger vertical velocity dispersion. The instability saturates when the system has reached a new, nearly isotropic configuration in velocity space. This picture has been confirmed by more recent simulations with much higher resolution and physical complexity [59]. As it reaches a new, nearly isotropic configuration, the system undergoes a transition from a cold disk into a spheroid. This mechanism has indeed been proposed as a possible channel for the formation of bulges starting from cold stellar disks [60].In simulations of disky dwarfs on eccentric orbits interacting with a Milky-Way-sized halo, the following sequence of events is typically observed. First, tidal shocks induce strong bar instabilities in otherwise stable, light disks resembling those of present-day dIrrs. Second, the bar buckles due to the amplification of vertical bending modes and turns into a spheroidal component in disks with relatively high stellar surface density (Mayer et al.) [13, 14], or else subsequent shocks destroy the centrophilic orbits supporting the bar which then loses its elongation and heats up into a more isotropic diffuse spheroid [39, 41]. An example of the first channel of transformation is shown in Figure 2 (top). The second channel for the transformation is favored in systems with lower mass, lower surface density disks, for these tidal heating is particularly efficient because the dynamical response of the stellar system is impulsive rather than adiabatic. As shown in Mayer et al. [41], the latter conditions likely apply to the progenitors of the faintest classic dwarf spheroidals (dSphs) such as Draco, Sculptor or Leo I, or the And satellites of M31, while the bar-buckling sequence might have been more likely for the progenitors of the brightest dSphs such as Fornax and Sagittarius, and even more so for those of the bright dwarf elliptical satellites (dEs) of M31, such as NGC185 and NGC167 (but not M32 whose unusually high surface density for a dwarf suggests that it is the “threshed” core of a low luminosity elliptical–see Bekki 2001. The bar-buckling sequence of instabilities also occurs for the progenitors of bright dwarf spheroidals and dwarf S0s in galaxy clusters, where both tidal stirring and harassment, that is, repeated flybies with the brightest cluster members, are at play [61]. Tidal heating/tidal mass losses remove the disk outside the region that goes bar unstable. Removal of the outer region, which contains most of the angular momentum in the original disk, can be complete or partial, depending on the number and strength of tidal shocks. Within this scenario, the LMC and SMC, and perhaps the two bright dEs of M31 which show fairly elliptical outer isophotes, are in earlier stages of the transformation, but may also be sufficiently massive and dense to limit the tidal damage and never end up into spheroidals [14]. Some of the faint dSphs, that show markedly elongated isophotes, such as Ursa Minor and some of the newly discovered ultrafaint dwarfs (e.g., Bootes; see [62], and Leo V; see [63]), may owe such elongation to a residual bar-like component rather than to tidal deformation.Figure 2
Top: color-coded logarithmic density maps of a tidally stirred dwarf seen face-on (i.e., with the line-of-sight perpendicular to the initial disk orientation, on the top) and edge-on (i.e., with the line-of-sight parallel to the initial disk orientation, on the bottom). The time increases from the left to right; each snapshot is separated by about half an orbital time (the orbital time is~2 Gyr in this simulation), starting with the time corresponding to the first pericenter passage, when the bar first appears. Boxes are 10 kpc on a side. The edge-on view shows clearly the buckling of the bar occurring on the second orbit, and the subsequent transformation into a diffuse spheroidal. Bottom: gray-scale surface brightness maps of the remnant of the simulation shown after 10 billion years of evolution (about 5 orbits). Two perpendicular viewing projections are shown. The limiting B band surface brightness shown in the images corresponds to μB=32 mag arcsec-2, and a B band stellar mass-to-light ratio of 5 was adopted for converting surface mass density into surface brightness (see [14] on models for the evolution of the luminosity and stellar mass-to-light ratio in the tidally stirred dwarf). The faint simulated remnant resembles classic dSphs such as Draco or Carina in both apparent shape and luminosity and surface brightness distribution.Evolution of structural parameters of a tidally stirred dwarf in a high resolution numerical simulation. The plot shows the results for one of the models studied by Klimentowski et al. [39], whose initial disk was oriented at 90 degrees with respect to the orbital plane (this is a conservative case since other orientations leave almost no residual angular momentum, see text in Section 3). Upper panel: the maximum circular velocity (solid line, left axis) and the radius at which the maximum circular velocity occurs (dashed line, right axis). Middle panel: the velocity dispersion (total 3D, and 1D along three different cylindrcal axes) expressed in units of the maximum circular velocity (indicated as Vpeak in the text). Lower panel: evolution of the ratio of the mean rotation velocity to the total (3D) velocity dispersion and the angle γ between the total angular momentum vector of the stars and the orbital plane (dashed line, right axis). In all panels vertical dotted lines indicate pericentre passages. Loss of angular momentum due to tidally induced instabilities and simultaneous increase of stellar velocity dispersion owing to tidal heating lead to a low v/σ ratio comparable to that of dSphs. See Klimentowski et al. [39] for details on how internal angular momentum is lost.
(a)(b)(c)It is important to stress that tidal stirring operates independently of tidal mass loss of the baryonic component. While systems that undergo substantial tidal mass loss are also effectively transformed, the transformation can occur even when stellar tidal mass loss is marginal (see, for example, the GR8 model presented in Mayer et al. [13, 14]). This implies that the detection of tidal tails in dSphs should not be used as a direct way to test the feasibility of tidal stirring. Instead, the deep structural analysis of dSphs and also of the socalled transition dwarfs, a class with intermediate properties between dSphs and dIrrs [15], offers a much better test of the predictions of tidal stirring for the different stages of the transformation mechanism. In clusters, the discovery of disk-like features and bars in some dwarfs previously classified as dSphs [64] matches very well the expectations of the tidal stirring and harassment models. While in the Milky Way halo the main epoch of interaction between the primary and the satellite may be over, as suggested by the the Sagittarius stream that is the only bright stellar stream present today in the Milky Way halo, the study of other groups with more recent assembly histories may unfold a population of satellites in the process of being transformed.The remnants left behind by tidal stirring have nearly exponential profiles and very low surface brightness (Figure2). Tidal features typically lie at very low surface brightness levels, below 32 mag arcsec-2 (Figure 2). The brightest among the remnants, those coming from progenitors having relatively massive disks (>108M⨀) and high surface density disks, develop a central steepening of the profile during the bar stage that persists even after buckling, and overall their profile resembles that of the bright dwarf elliptical satellites of M31, like NGC205 [13, 14]. Most importantly, both “tidally heated” and “buckled” remnants have a very low angular momentum, consistent with what is seen in dSphs and dEs, despite being descendants of disk-like systems. The loss of angular momemtum is a by product of the bar instability. The bar sheds angular momentum outwards to the outer stellar disk and dark matter, which are stripped after repeated shocks, thus leaving behind a surviving stellar and dark matter core with very low rotation, having a typical final v/σ<0.5. The gradual loss of internal angular momentum and decrease of v/σ can be inspected in Figure 3. Some residual rotation may be present at the end depending on the initial structural properties and orbits of the dwarfs [13, 14]. Klimentowski et al. [39] have also shown that for the same inital disky dwarf model, the initial orientation of the disk angular momentum of the dwarf with respect to the orbit also matters. In orbits with high inclination, for example, polar orbits, v/σ~0.4, perhaps consistent with what is found in Leo I [65], as opposed to close to zero in coplanar or moderately inclined orbits. How likely is one or the other configuration in CDM? The answer still awaits us since it is likely that inclusion of the disk of the primary may have played a significant role, for example, by dragging satellites towards its orbital plane and thus yielding a preferential bias towards a coplanar configuration [66]. This would explain why most dSphs do not show sign of residual rotation. In Lokas et al. [67], we analyzed the velocity structure of the remnants. In some cases we find radial anisotropy in the velocity ellipsoid. This can be significant in remnants that have some residual rotation and are triaxial due to a residual bar-like structure in the remnant, or can be negligible in those that have been efficiently heated, turning into nearly isotropic spheroids with negligible rotation. In other words, when tidal stirring produces a good match to a dSph, anisotropy in the kinematics is not important.The transformation mechanism that we have studied requires the dwarf to be on a bound orbit; for the mean apocenter/pericenter ratio found in cosmological simulations,~5, Mayer et al. [14] determine that an apocenter distance comparable to the distance of Leo I (250 kpc), the farthest dSph satellite of the MW, is a limiting case for producing a dSph from a disky dwarf in less than 10 Gyr. However, this estimate is very conservative and should be revised. In fact,in the meantime we have learned that some satellites enter the primary system in subgroups and thereby might have already felt significant tidal perturbations before entering the primaries [24, 68]. Kravtsov et al. [24] find that, at least in some cases, most of the tidal heating in cosmological subhalos occurs before they enter the primary halo. Furthermore, we have assumed that the only thing that could affect the orbit of the dwarf within the primary halo is dynamical friction, and, moreover, that its effect can be neglected for the typical low masses of subhalos. While this would be a reasonable picture for dwarfs orbiting in a spherical, nonevolving primary halo, cold dark matter halos are triaxial and accrete mass via both smooth accretion and mergers. Triaxial halos are populated by families of chaotic orbits whose pericenters can fluctuate over time. Yet, baryonic infall makes the potential of the primary halo very close to spherical [69], which also agrees with current observational limits on the shape of the MW halo [70], thus suggesting that triaxiality should not be an important effect. Instead, dwarfs infalling at very early epochs, when the primary halo is still undergoing substantial growth via merging of relatively massive subgroups, might undergo rapid changes in their orbits as the global potential changes. Another effect, which is seen to take place in simulations, is orbit scattering via the interaction with another satellite, which can not only modify the parameters of the orbit of the satellites but even cause ejections when a three-body interaction takes place [71].All simulations conducted to study the dwarf-primary interactions neglect the effect of the disk of the primary. The disk of the Milky Way was likely in place already atz=1.5–2, hence during most of the time during which satellites were accreted and evolved within the primary halo. While the tidal effect of the disk is not expected to be important for typical pericenter distances of satellites accreted below z<1, because these should be larger than 20–30 kpc (see [14]), satellites accreting earlier had smaller pericenters that would graze the disk and could even be quickly reduced by the additional dynamical friction provided by the disk itself [72] if satellites accrete more frequently on a prograde rather than retrograde orbit [66, + in prep.]. D’Onghia et al. [73] find that disk shocking, namely, tidal shocks induced by passages through the disk, can affect significantly the evolution of satellites having masses <109M⨀ and pericenters <20 kpc, causing the disruption of a fraction of them and thus playing a role in the missing satellites problem (which normally neglects disk shocking) as well as in determining the radial distribution of satellites inside primary halos.This “tidal stirring” accounts for most of the similarities and differences between dIrrs and dSphs, including the existence of the morphology-density relation, by postulating progenitors of dSphs with light, low surface brightness disks embedded in massive halos. This, however, does not mean that such progenitors were identical to present-day gas-rich dIrrs. Indeed, since they formed at highz, they likely had assembly histories quite different from present-day dIrrs, and thus their stellar populations and metallicities were different (this is an aspect that will be addressed by new, ongoing simulations that start from a gas-rich dwarf galaxy formed self-consistently in a cosmological simulation). The next step would be to verify the model within a fully cosmological simulation, and thus extend the analysis directly to the implications for the star, formation and metallicity histories of the dwarfs. Unfortunately, to date cosmological simulations with hydrodynamics have not allowed a robust analysis of the structural evolution of satellites due to their limited resolution (typically the force resolution is of order a few hundred parsecs, see Mayer et al. [74] for a review, so the tiniest dSphs like Draco are not resolved at all). Satellites, in addition, are too bright and dense in published cosmological galaxy formation simulations due to numerical loss of angular momentum and overcooling [75]. Searching for evidence of tidal stirring in these simulations is thus quite hard, but it can be done in a qualitative sense for a few well-resolved dwarfs. We selected the brightest satellites (MB>-14) of the large spiral galaxy in the cosmological hydrodynamical simulation of Governato, Mayer et al. [76], as well as similarly bright dwarfs outside the virial radius of the same galaxy. Figure 5 shows their v/σ within the effective radius versus the number of orbits performed within the main system. Clearly v/σ correlates well with the number of orbits as expected within the tidal stirring scenario. We also found that the shape of the stellar components of the dwarfs goes from more disky to more spheroidal with increasing number of orbits. The absolute values of the v/σ have to be taken with caution because numerical two-body heating (e.g., Mayer [76]) is certainly an issue for these objects (halos have only a few thousand particles at this scale). However the trend is evident. A similar result, more recently, has been obtained in a much higher-resolution cosmological simulation of the formation of a massive early-type galaxy (Feldmann et al., in prep.) as well as in newer, higher-resolution simulations of the formation of a Milky-Way-sized galaxy (Callegari et al., in prep.).


## 4. Tidal Tails in Disky Dwarfs and Line-of-Sight Stellar Velocity Dispersions

As the dwarf is tidally perturbed and gradually transforms into a dwarf spheroidal, it also loses mass. In Mayer et al. [18] tidal mass loss and the formation of tidal tails in dark-matter-dominated, tidally stirred disky dwarfs was studied using a range of initial models embedded in an NFW halo and a range of cosmologically motivated orbits, that is, spanning and apocenter-to-pericenter ratio of 3 to 10. The main conclusions were that (1) tidal tails projecting along the line of sight could lead to an overestimate of the velocity dispersion (and thus an overestimate of the mass-to-light ratio) by at most a factor of 2 and (2) the most important contribution to the measured mass-to-light ratio is always the intrinsic dark-matter content of the dwarf. The corollary of the second point is that the most dark-matter-dominated dwarfs have the faintest tails, just lying at the detection limit of photometric surveys. However, the role of projections effects, especially how likely tidal tails lie perpendicular to the observer and thus can be more easily detected, was not clarified. Klimentowski et al. [57, 77] and Lokas et al. [65] confirmed, in a much more detailed study, that velocity dispersion profiles in dSphs can be affected by contamination from unbound stars in the tails. While the central velocity dispersion is not changed (the contamination from unbound stars is statistically too weak since most of the stars projected towards the inner core of the dwarfs are indeed bound), the outer velocity dispersion can increase by nearly a factor of 2, with consequences on the measurements of the total mass and mass-to-light ratio of the dwarf. The same authors present a method of interloper removal to clean observed samples from unbound stars contamination. In Klimentowski et al. [78] tidal tails disky dwarfs were revisited. The interesting conclusion is that on typical cosmological orbits (apocenter/pericenter ~5-6), tails point towards the observer for the largest fraction of an orbital revolution of the dwarf within the Milky Way halo, especially where it spends most of the time, namely, near apocenter. This renders the detection of tails extremely difficult and maximizes the enhancement of the line-of-sight velocity dispersion because it implies that unbound stars belonging to the tails would be normally projected along the line-of-sight, contaminating observed samples, although the effect is complicated by variations in the intrinsic line-of-sight velocity dispersions along the different axes of the dwarfs, see [57, 77]. The difficulty in separating the tails from the bound core of the dwarfs due to this biased projection effect may explain why in only a few of the dSphs, for example, Carina [79] and Ursa Minor [80], tails have been tentatively detected. This effect adds to the most important requisite for tidal tail detection, namely, the need of an exceptional photometric technique [81].


## 5. Gas Stripping; Ram Pressure, Tides, and the Cosmic Ultraviolet Radiation

Mayer et al. [14] showed that tidal stripping alone cannot produce the low gas fractions found in dSphs starting from a gas-rich disky dwarf. Bar instabilities drive gas towards the center, making it tightly bound. Such inner gas distribution is not stripped by tides for the same reason of why an inner stellar core always survives in the tidally stirred dwarfs, namely, because its binding energy is too high and the response to tidal shocks is nearly adiabatic. Gas consumption by star-formation does not solve the problem if one adopts the mean star formation rates inferred for dSphs [2, 4]; too much gas is left even after billions of years [14]. In addition, gas turning into stars during the orbital evolution gives rise to an extended star formation history, a feature that is seen only in a subset of dSphs [3, 15]. Therefore a mechanism that selectively removes the gas while leaving the stars unaffected seems required. Mayer et al. [20] studied the combined effect of ram-pressure and tidal stripping. Ram pressure-stripping occurs when the pressure force exerted by the ambient gaseous medium exceeds the gravitational restoring force felt by the gas inside the dwarf. The ram-pressure is given by Pram=ρghVorb2, where ρgh is the density of the ambient halo gas and Vorb is the orbital velocity of the galaxy (Gunn & Gott 1972). Assuming a constant ram pressure, there will be a characteristic radius at which the ram pressure force Frp=PramSgd (where Sgd is the surface area of the gas disk) is equal to the gravitational restoring force Fgr(r)=∇ϕ(r), where ϕ(r) is the gravitational potential of the galaxy. The gravitational restoring force will indeed vary with radius since in galaxies the potential is a function of radius. Since the gravitational restoring force will increase with decreasing radius in a typical galactic potential (e.g., see Abadi et al. 1999) the gas located at or outside the radius at which Frp=Fgr will be stripped.Mayer et al. [20] constructed two-component models for the Milky Way halo in which a dark matter halo consistent with the results of ΛCDM simulations has an embedded diffuse gaseous component with a temperature of ~106 K and a density of about ~10-4 atoms/cm3 at 30 kpc from the center, consistent with the values inferred from OVI absorption measurements and the existence of the Magellanic Stream [82]. Dwarf galaxies are placed on eccentric orbits (apo/peri= 5-6) with pericenters of 30 or 50 kpc. The initial models were gas-rich disky dwarfs (Mgas/Mstars≥0.4). It was found that ram pressure increases by a factor up to 10 the amount of stripped gas mass compared to the case in which only tides are considered (Figure 4). Ram pressure strongly depends on the depth of the potential well of the dwarfs. While for dwarfs with Vpeak≤30 km/s most of the gas content is easily removed, for more massive dwarfs the end result depends a lot on the orbit and on gas thermodynamics (the effect of thermodynamics is seen in Figure 4, where we compare results for an adiabatic run, a run with radiative cooling, and one with both radiative cooling and the cosmic ionizing background).Figure 4
Time evolution of the bound gas mass for a disky dwarf galaxy model(initialVpeak=42) km/s within a Milky-Way-sized dark matter halo (Mvir∽1012M⨀) having a hot gaseous halo about 1% of its total mass (see [20] for details on the modeling). The dwarf's orbit has an apocenter of 150 kpc and a pericenter of 30 kpc. The same model has been run with adiabatic gas conditions (thin solid line), radiative cooling with no heating (thick solid line), and radiative cooling plus heating by the cosmic ionizing UV background (dashed line), assuming that when the simulation is started, the time corresponds to z=2. The long-dashed line shows the results for a run in which the hot gaseous halo of the Milky Way was absent to isolate the effect of tides from that of ram pressure. Stripping from ram pressure only is instead shown by the thick solid with dots; in this run, the same dwarf model was evolved in a “wind tunnel”, moving with a speed comparable to the orbital velocity at pericenter in the other runs. In the “wind tunnel” the dwarf moves within a static gas distribution along a straight trajectory withe specified velocity (periodic boundary conditions are used for the gaseous background), but responds only to the ram-pressure force. The latter curve spans less than a Gyr of evolution since ram-pressure stripping saturates quickly without tidal mass loss.Figure 5
v/σ as a function of the number of orbits for the satellites in the cosmological hydrodynamical simulation of Governato, Mayer et al. [56]. v/σ is measured within the half mass radius of the dwarfs at the end of the simulation, namely, after 13 billion years of evolution. The mean number of orbits for each of the three groups of dwarfs appears on the horizontal axis.For a galaxy moving on a noncircular orbit, the ram-pressure is not constant but varies with time as both the galaxy's orbital velocity and the density of the ambient medium change along its trajectory within the primary. The pericenter distance sets the maximum strength of the ram-pressure force sincePram=ρghVorb2, and both ρgh and Vorb are maximum at pericenter. Moreover, there is another important time-dependent effect for galaxies on eccentric orbits. Repeated tidal shocks lower progressively the depth of the potential well of the dwarf at each pericenter passage, reducing the gravitational restoring force, and thus allowing gas removal towards increasingly smaller radii as time advances (this would be the case even if the ram-pressure wind was constant). This explains why ram pressure stripping can continue over several billion years (Figure 4) rather than saturating after the first pericenter passage. However, when gas can cool down radiatively but cannot be heated, the stripping process saturates after two orbits; this is because the gas torqued by the bar flows towards the central region of the dwarf, increasing its central density and rendering the response of the potential to tidal shocks more adiabatic (see Section 7).In principle stripping may still occur after the saturation induced by the bar inflow via a mechanism that is not correctly captured by the SPH simulations discussed throughout this paper, namely, turbulent stripping by ablation due to Kelvin-Helmoltz instabilities at the interface between the gas in the dwarf and the surrounding hot diffuse halo ([83, 84], but see how simple modifications of standard SPH can solve the problem in [85]). In hydrodynamical flows two shearing fluids moving with relative velocity Vrel are subject to an instability (the Kelvin-Helmoltz instability) that tends to ablate their interface; a wave-like perturbation will grow proportionally to the density contrast and relative velocity of the fluids, but could be damped with increasing viscosity or if an external force, such as a gravitational field, is applied to the system.We can show that Kelvin-Helmoltz instabilities will not occur for dwarfs embedded in a massive dark halo because of the stabilizing effect of the gravity of the halo. We neglect the effect of SPH artificial viscosity in the following calculation; this is a conservative assumption since viscosity would stabilize the system further. Following existing analytical predictions [83], we estimate that the critical value of the gravitational acceleration necessary to stabilize the dwarf gas disk against Kelvin-Helmoltz in dwarf galaxy models with Vpeak=40 km/s used in Mayer et al. [20] and Mayer et al. [41] is gcr~0.1 initially, where gcr=2πV2/DRg (V~200 km/s is the average orbital velocity of the galaxy, Rg=0.5 kpc is the scale length of the gas component, and D=ρg/ρgh is the ratio between the density of the gaseous disk at R~Rg and the time averaged density of gaseous halo along the orbit of the dwarf; and for simplicity we express the gravitational acceleration in the adimensional system of units of our simulations, in which we assume G=1 for the gravitational constant G ). The self-gravity of the dwarf galaxy within Rg, which is mainly provided by the dark halo, is instead g~2.5>gcr, where g=GMhalo/Rg2. We note that g>gcr holds down to about 1/5 of the disk scale length, and also for R>Rg. Hence the gaseous disk of the dwarf is initially stable to Kelvin-Helmoltz instabilities. However, on subsequent orbits the situation can change. For the simulation presented in Mayer et al. [41] after the second pericenter passage, the density of the dwarf within 0.5 kpc, decreases by a factor of 4 as a result of the tidal shocks, so that g drops to ~0.6 at one disk scale length, now being very close to gcr (the latter has also decreased in the meantime, gcr~0.3, since the mean density of the gas has dropped). The gas component of the dwarf is now only marginally stable to Kelvin-Helmoltz instabilities, but using the formula to calculate the mass loss rate due to Kelvin-Helmoltz [83] for Rg=0.5 kpc one derives a characteristic stripping timescale still quite long, that is, comparable to the Hubble time.There is then one more stripping mode to examine. Although formally standard SPH solves the equations for an inviscid fluid,  de facto the necessity of artificial viscosity renders the fluid model viscid. It thus makes sense to consider laminar viscous stripping as another possible stripping mechanism. The mass loss rate in this case is given byṀ~12/2.8πRg2Vrelρgh(λmax/Rg)(c1/Vrel) [83, 86], where λmax is the longest wavelength not stabilized by gravity. Assuming that, at second pericenter, the longest unstable wavelength is λmax~0.5 kpc, one obtains a laminar viscous timescale of ~2 Gyr for the typical ambient gas densities and relative velocities in our simulations (Vrel=Vorb). The gas is indeed completely stripped ~1 Gyr later in cases in which the gas component remains diffuse and extended because cooling is inefficient (e.g., the run with adiabatic gas and with added cosmic UV background presented in Figure 4; see also next paragraph). In runs where only radiative cooling is considered, the longest unstable wavelength is much smaller than the radius of the residual gas, which implies a laminar viscous timescale close to the Hubble time. This explains why the gas is not completely stripped in cooling-only runs (see Figure 4). In conclusion, despite the strongly time-dependent behaviour of all the variables involved in the problem, both the action and the saturation of stripping seen in the simulations is consistent with the expected characteristic timescales and relative importance of the various ram-pressure stripping modes.The next point to discuss in order to understand the different mass loss curves shown in Figure4 is the effect of radiation physics/thermodynamics, which we have just hinted during the description of the stripping process above. The temperature evolution determines whether the gas component stays extended or becomes concentrated in the central, deeper part of the potential well as a result of tidally induced bar-driven inflows. Compression from the outer medium heats the gas. The gas is rapidly heated to 105 K, where the cooling function peaks (the initial temperature of the gas disk in the dwarf models is in the range ~3000–8000 K depending on the initial mass and is set by hydrostatic equilibrium requirements) at which point it cools radiatively to 104 K in a fraction of a dynamical time; such cold gas easily sinks towards the center due to the torque exerted by the bar and cannot be removed by ram pressure. Instead, if compressional heating is not radiated away, as when the gas evolves adiabatically, the increased pressure opposes the bar-driven inflow, keeping more gas at larger radii where it can easily be stripped. For stripping to be very effective for dwarfs with initial Vpeak~30–60 km/s, it is sufficient that the temperature of the gas is kept above 104 K (the virial temperature of these halos is 3–5×104 K). This requires some heating source to counteract radiative cooling. Mayer et al. [20] find that for Vpeak~30–40 km/s such temperature increase can be achieved owing to heating by the (uniform) cosmic UV background at z> 1.5–2, where the heating rate and ionizing flux rates are based on standard models for the time evolution of the intensity of the cosmic ionizing background [49, 2000].For even higher values of the circular velocity (Vpeak~40–60 km/s), complete stripping would require an even higher heating rate. This is likely to be provided by the local ionizing radiation originating from the primary galaxy (the Milky Way or M31 for the case of the Local Group). Mashchenko et al. [87] calculate that the FUV flux of M31 derived from its Hα luminosity is higher than these of the present-day value of the cosmic UV background out to 10–20 kpc from its center. Current starbursts have FUV luminosities 103–104 higher than the MW and M31, in the range 1044–1045 erg/s [88]. According to cosmological simulations at z= 2-3 Milky-Way-sized galaxies were hosting a major central starburst, forming stars at a rate of ~20–30M⨀/yr [75, 89]. This is consistent with the star-formation rates measured for z=2 galaxies that should evolve into L* galaxies by the present epoch (Conroy et al. 2007). Determining the escape fraction of ultraviolet photons that will contribute to heating and ionizing, the gas of the dwarf is a complex task, with the estimated escape fraction varying between a few percent to more than 10% (e.g., Fernandez-Soto et al. [90], Shapley et al. [91]). We choose a simpler approach by assuming that the FUV luminosity of the primary galaxy in the starbursting phase is comparable to that of a major present-day starburst (LFUV=1045 erg/s). At higher redshift, dust absorption should be lower since the metallicity should also be lower, thereby our estimate, while crude, should be on the conservative side. Under this hypothesis we obtain that at 30 kpc from the center the heating rate was 10 times higher than that associated with the metagalactic UV background at z~2. We have run new simulations including such a local, time-dependent UV background (the intensity of the flux is modulated by the orbital distance of the dwarf) and found that ram-pressure stripping is greatly enhanced, leading to complete gas removal after a couple of orbits even for Vpeak~50 km/s [19]. A systematic exploration of the effect of the local ionizing radiation over a range of mass scales of dwarf galaxies will help assess the overall relevance of the effect in the context of the evolution of dwarf galaxy satellites.The implications of these simulations on the enhanced gas stripping resulting when the ionizing background at high redshift is taken into account are quite important. Indeed we can argue that if the progenitors of Draco or Ursa Minor fell into the Milky Way atz>1.5–2,then ram pressure combined with tides was able to remove their entire gas content in a couple of orbits. This translates into a timescale of about 2-3 Gyr after infall assuming a range of orbital times consistent with their current distance from the Milky Way. Therefore, in this scenario the observed truncation of the star formation in Draco and Ursa Minor more than 10 Gyr ago occurred as a consequence of the infall of these galaxies into the Milky Way halo. Draco would have formed most of its stars before infall since most of the gas becomes ionized while approaching pericenter for the first time. This scenario, however, would still be unable to explain the very high dark matter content of a galaxy like Draco nor why do other dSphs, such as Fornax, appear to have a similar total mass (baryons plus dark matter) but a much lower dark matter content. We will see in the next section that these other properties of dSph satellites of the Milky Way can also be explained once proper assumptions on the structure of their disky progenitors are made, and the time-dependent nature of the cosmic ionizing background is taken into account.


## 6. A Scenario for the Origin of Classic Dwarf Spheroidals in a Hierarchical Universe: The Timing of Infall into the Primary

In Mayer et al. [41] we built on the results of the previous section and we proposed a coherent scenario that explains at the same time the origin of the common properties of dSphs (low gas content, exponential profiles, low luminosity and surface brightness, and low angular momentum content) and their differences (different star-formation histories and mass-to-light ratios). In this model the key parameter is the epoch of accretion onto the Milky Way and a key assumption is that the progenitors of present-day classic dSphs were not simply gas-rich but extremely gas dominated, consistent with what is found in most present-day dIrrs in the Local Group and elsewhere in the nearby Universe [92]. The large gas fractions found in field dwarfs can be understood in terms of a decreasing star-formation efficiency towards decreasing galaxy mass. Recently, the THINGS survey [93] has confirmed that disky dwarfs have a star-formation efficiency, defined as the fraction of gas (atomic+molecular) that is converted into stars, well below that of normal spirals, of order 1% or less. The low gas surface densities typically found in dwarfs likely imply a low conversion efficiency between atomic hydrogen and the star-forming molecular hydrogen phase [94], probably explaining the low star-formation efficiency (note that the conversion between molecular gas and stars does not seem to be lower in dwarf compared to normal spirals, see [95]). Such conversion can be even less efficient in presence of the ionizing ultraviolet flux arising during reionization, which can dissociate molecular hydrogen [94]. Therefore for field dwarfs that were accreted by the Milky Way or M31 at z>1, the assumption of mostly gaseous baryonic disk is even more well grounded.The initial conditions, including the orbits of the satellites, were chosen based on a hydrodynamical cosmological simulation of the formation of a Milky-Way-type galaxy [75]. We found that satellites that were accreted when the cosmic ionizing background was still high, roughly before z=1, were completely ram pressure stripped of their gas in one to two pericenter passsages (Figure 6). As a result their star formation was truncated. As explained in Section 5, the effect of the ionizing radiation is to heat and ionize the gas, making it more diffuse because of the increased pressure support, and to suppress star formation. This, in turn, makes it easier to strip even from the central regions of the dwarf, essentially having the same effect of a reduced binding energy. Hence gas-rich dwarfs accreted when the UV radiation background was at its peak lost most of their baryonic content because this was initially in gaseous form, thus naturally ending up with a very low luminosity. While their baryonic content dropped orders of magnitude below the cosmic mean as a result of gas stripping, their original central dark matter mass in the central region around the surviving baryonic core was largely preserved because dark matter is affected only by tides, not by ram pressure. This automatically produced very high mass-to-light ratios, of order 100 (see Mayer et al. [80, Figure 2]). We showed that all the final properties of such systems after 10 billion years of evolution, including the stellar velocity dispersion profiles, resemble those of the classic strongly dark-matter-dominated dwarfs such as Draco, Ursa Minor, or And IX. Even the brightest among the ultrafaint dwarfs, that have velocity dispersions >5 km/s (e.g., Ursa Major) may be explained by this model. However, the very low characteristic mass scale of most ultrafaint dwarfs suggests that other formation paths might indeed be more likely (see Section 8). Dwarfs that fell into halos of bright galaxies below z=1, when the cosmic UV radiation dropped by more than an order of magnitude, retained some gas because tides and ram pressure could not strip it completely and underwent subsequent episodes of star formation at pericenter passages due to bar-driven inflows and tidal compression [13, 14]. These ended up in dSphs that are brighter for a given halo mass (or given central stellar velocity dispersion) compared to the ones that were accreted earlier. This should be case with, for example, Fornax, Carina, or Leo I. The two regimes of infall epochs explain why Fornax and Draco have roughly the same halo peak circular velocities (and thus mass) despite having a luminosity and mass-to-light ratio that differ by about an order of magnitude. Likewise, Carina and Leo I, these being prototypical cases of dSphs with an extended (episodic) star-formation history, have a luminosity comparable to Draco but a mass-to-light ratio 5–10 times lower than that of Draco [1].Figure 6
Evolution of the gas-dominated disky dwarf model studied in Mayer et al. [41], which produces a dark-matter-dominated dwarf resembling Draco after 10 Gyr of evolution. This N-Body + SPH simulation employed millions of dark matter, gas, and star particles. It included tidal mass loss due to a live Milky Way halo, ram-pressure stripping in a tenuous gaseous halo, radiative cooling, and a time-varying cosmic ionizing UV background consistent with the Haardt and Madau (2000) model. The snapshots show the color-coded logarithmic density maps (the brighter the color, the higher will be the density, with densities in the range 10-32-10-23 g cm–3) for the first 2.5 Gyr of evolution. Boxes are 30 kpc on a side. The dwarf begins falling into the Milky Way halo on a typical eccentric cosmological orbit (apo/per=5 at the beginning of the simulation, which corresponds to z=2). At the first pericenter passage (Rperi=30 kpc) a prominent ram-pressure tail is evident (top left), and once the dwarf comes to first apocenter (top right), it has lost already more than half of its gas. As it begins the second orbit, ram-pressure stripping continues to remove gas (bottom left), until all gas is stripped at second pericenter (bottom right).As a final remark, we note that Madau et al. [38] argue that a very low efficiency of star formation, corrresponding to less than 0.1% of their total mass being converted into stars, would offer a solution to the excess in number counts of subhalos with Vc>20 km/s in dark-matter-only simulations (see also [78] for a similar interpretation). Our model for the origin of Local Group dwarf spheroidals provides a clue to why dSphs were so inefficient at producing a stellar component, thus pointing to a solution of the substructure problem at the bright end of the mass function of dwarf satellites of the Milky Way, which essentially contains all the classic dSphs. Instead of relating the low efficiency of star-formation to photoevaporation and/or suppression of gas accretion by the cosmic ultraviolet background, we argue that it arose naturally from intrinsic low star-formation efficiency in the progenitor gas-rich dwarfs (well below 1%) combined with copious gas stripping after they were accreted in the potential of the primary galaxy. Our mechanism is absolutely general in hierarchical structure formation and should thus apply to dwarf galaxy satellites of any galaxy group. The combination of an intrinsic low star-formation efficiency prior to infall with ram pressure and tidal stripping can be thought of as an effective feedback mechanism alternative to reionization and supernovae feedback. Recent models that relate star-formation directly to the formation of molecular hydrogen and to its dependence on metallicity [96, 97] show convincingly that the star-formation efficiency was at the low levels assumed by us, and invoked by Madau et al. [38], when the metallicity was below 0.1 of the solar value. This is because both molecular hydrogen formation and self-shielding from the dissociating UV radiation depend on the dust content, which drops with decreasing metallicity. Interestingly, the current metallicity dSphs, both of the ultrafaint ones and of the classic ones, is comparable to or smaller than a tenth of the solar value [52], suggesting that these objects likely spent a significant fraction of their assembly history at metallicity lower than such critical threshold. Therefore inefficient star formation played a key role in delivering gas-dominated dwarfs at the time of their infall into the halo of the primary and at the same time is key to understand the missing satellites problem.


## 7. The Interplay between Gas Stripping and the Tidally-Induced Transformation of the Stellar Component

The removal of gas due to ram pressure can in principle have effects on the dynamical evolution of the other components of the dwarf, dark-matter and stars, since it is initially a nonnegligible fraction of the total mass within the central kiloparsec. We have performed a number of tests to explore in detail the nature of the transformation of the baryonic component in the simulations presented by Mayer et al. [41], where both stars and gas are present in the initial disky dwarf. The main goal was to determine the relative role of the rapid removal of the gas (Figure 6), which comprises most of the baryons initially, and that of the repeated tidal shocks in changing the shape of the stellar component. Although the initial dwarf model is dark matter dominated by construction, baryons comprise as much as 30% of the total mass within the initial exponential disk scale length. Their rapid removal due to ram-pressure stripping might in principle affect the dark matter potential, possibly lowering its density as found in previous studies where baryonic stripping occurs as a result of powerful supernovae winds [98–100].Figure7 shows principle axis ratios s=b/a and q=c/a (a>b>c) of stars, calculated from the eigenvalues of a modified inertia tensor [101]: Iij=∑αxiαxjα/rα2, where xiα is the i coordinate of the αth particle, rα2=(y1α)2+(y2α/s)2+(y3α/q)2, and yiα are coordinates with respect to the principle axes. We use an iterative algorithm starting with a spherical configuration (a=b=c) and use the results of the previous iteration to define the principle axes of the next iteration until the results converge to a fractional difference of 10-2. Results are shown for three experiments. The comparison between the red and the black lines clearly shows that repeated tidal shocks are necessary for the transformation of the stellar component to occur; c/a increases by more than a factor of 6 when the dwarf is continuously tidally shocked relative to a case in which it just loses most of its baryons owing to ram pressure and then evolves without any tidal perturbation (in the latter case we removed the primary halo from the simulation after the gas was stripped). The green lines in Figure 7 show a test in which about 30% of the initial gas content is retained until the end because the UV background is absent and thus the effect of ram pressure is reduced (we tested that not including the cosmic UV background at all or including it with the low amplitude expected at z<1 from the Haardt and Madau model yields the same result, see Mayer [19] and Mayer et al. [20]). The residual gas is funneled to the center by the bar, where it forms a very dense knot [20]. We notice that despite the fact that this is a small fraction of the initial gas content, it represents a nonnegligible contribution to the central potential because it all ends up in the inner 0.5 kpc (corresponding to the initial disk scale length). In this case the dwarf maintains a bar-like, prolate shape even after 10 Gyr, hence the lower c/a. After 5 Gyr the central density is 8 times higher compared to the simulation in which complete gas stripping occurs. As a result tshock>torb within 0.5 kpc, where tshock is Rperi/Vperi, Rperi and Vperi being, respectively, the pericentric distance and the velocity at pericenter, and torb is the orbital time at 0.5 kpc from the center of the dwarf; the response of the system to the tidal forcing is thus adiabatic instead of impulsive, hence further morphological changes are inhibited. This demonstrates that while gas removal does not drive the transformation, it represents a crucial step for the evolution of the stellar component because the effect of the tidal shocks is considerably weakened when a dense central gas component is retained.Shape evolution of the stellar component. The upper panel shows the intermediate-to-major axis ratio,b/a, and the bottom panel presents the minor-to-major axis ratio, c/a. Solid lines correspond to the self-consistent simulation in which tides, ram pressure stripping, and UV background were included throughout the orbital evolution of the dwarf. Dotted lines correspond to the case where the dwarf galaxy was extracted from the simulation just after the gas was removed and evolved in isolation. Dashed lines show results of a test in which approximately 30% of the initial gas mass remains in the galaxy because the absence of the UV background reduces significantly the effectiveness of ram pressure stripping. Thick and thin lines correspond to 10 and 5 Gyr of orbital evolution, respectively (for the extracted dwarf we only show the result after 10 Gyr). The shape of the stellar component changes gradually over time and the presence of UV heating is essential for the shape transformation of thedwarf.
(a)(b)Figure7 also shows that c/a does not grow beyond 0.2 in isolation, even after a few Gyr of evolution. The average (apparent) ellipticity measured for late-type dIrrs in the Local Group is larger, ~0.58, for the 8 dwarfs having a range of rotational velocities comparable with those of our initial dwarf galaxy model (Vpeak~30–40 km/s) [1]. Similar values are found for dwarf irregular galaxies in clusters [102]. However, comparing with observed values of ellipticity one must take into account inclination effects, since the c/a discussed for our simulated dwarf is the intrinsic value, that is, the value that would be measured by an observer viewing the dwarf exactly edge-on. By viewing the dwarf at inclinations in the range 30–60 degrees, which statistically are a much more representative situation, the mean apparent c/a varies in the range ~0.4–0.7 within 3 disk scale lengths (it is 0.55 at 45 degrees of inclination), hence perfectly consistent with the observed values. This indicates that initial conditions used in tidal stirring experiments are a reasonable match to gas-rich dIrrs.To summarize, these experiments indicate that the repeated tidal shocks in the impulsive regime drive the transformation of the shape and mass distribution of the dwarf galaxy, and that gas removal is a necessary condition for them to be effective. Prolonged impulsive tidal heating is one of the ways by which tidal stirring can induce the morphological transformation from disk into spheroid, the other being bar-buckling (see Section3). The former is naturally favored for low mass, low density stellar disks that are naturally prone to an impulsive response and also less self-gravitating, while the latter is favored at higher stellar densities and thus higher self-gravity since it is based on the growth of unstable modes [14, 61].


## 8. The Ultrafaint Dwarfs in the Tidal-Stirring Scenario

In the last five years deep photometry with the Sloan Digital Sky Survey (SDSS) has unveiled a new class of ultrafaint dwarfs with structural properties (e.g., low angular momentum, no gas content) analogous to classic dwarf spheroidals (dSphs) but with masses and luminosities 1-2 orders of lower magnitude [17, 51, 52, 103] Indeed with velocity dispersions in the range 2–6 km/s and luminosities in the range -2<MB<-7, these objects are fainter than most known Globular Clusters, but clearly differ from them because of their lower stellar surface densities, larger optical radii, and much higher mass-to-light ratios. The dozen ultrafaint dSphs detected so far all have M/L~100–1000, hence they are even more dark matter dominated than the darkest among the classic dSphs, such as Draco and Ursa Minor. Like most classic dSphs, they are found at distances well within the virial radius of the Milky Way halo (at galactocentric distances <300 kpc). The brightest of them, such as Ursa Major, may be the product of the same transformation mechanism elucidated in the previous sections. In this case the initial progenitor managed to form just a minuscule stellar component before ram pressure aided by the UV background removed most of the baryons. But the low masses inferred for most of the ultrafaint dwarfs are below the critical mass threshold for “surviving” reionization ([104], Bullock, Kravtsov & Weinberg 2001, [12, 105]); they would have been below the threshold even before being accreted by the Milky Way assuming a factor of 2-3 decrease in their peak velocity dispersion/circular velocity (thus a factor ~8–30 in mass) due to tidal mass loss over billions of years. This implies that at z~7–12, when reionization began, they could not hold onto their gas and form stars, rather they suffered complete photoevaporation. The most plausible explanation for the origin of the ultrafaint dwarfs is that they formed their stellar components entirely before the onset of reionization (later gas accretion at z>1 would be difficult with such shallow potential wells). They are thus the natural candidates for being the “reionization fossils” predicted in the models of Ricotti and Gnedin [106] and Gnedin and Kravtsov [107]. High-resolution cosmological simulations of galaxy-sized halos indeed find about a thousand subhalos with virial masses >106M⨀ prior to reionization, hence massive enough for cooling via molecular hydrogen to lead to gas collapse and star formation before they are accreted onto the primary galaxy [108]. A low intrinsic efficiency of star formation due to inefficient formation of molecular hydrogen is expected for these low mass, low metallicty systems (see Section 6). In addition, even modest star formation would strongly affect these systems via supernovae feedback, keeping the star-formation efficiency low [100]. Inefficient star formation might thus be the main cause of the extremely low stellar content of the ultrafaint dwarfs. Moreover, gas photoevaporation owing to the rising ionizing background would remove most of their gas, hence most of their baryons, leading naturally to very high mass-to-light ratios without the need of additional environmental processes such as ram pressure and/or tidal stripping.On the other end, with original masses likely below107M⨀, up to two orders of magnitude less than those of classic dSphs, tidal stirring and tidal mass loss were also very effective in the progenitors of ultrafaint dwarfs. What we detect today is probably the surviving inner core of the original dwarf, which responded more adiabatically to the tidal shocks owing to the high halo concentration/central density expected in very low mass satellites [34, 69, 109]. However, such tiny subhalos were likely never disky in the first place. In fact for standard values of spin parameters expected in cosmological halos, their initial angular momentum content was too low to provide more support than thermal pressure against the low gravity of their tiny halo potential wells, especially in the presence of the cosmic ionizing UV background [77]. Therefore ultrafaint dwarfs do not owe their current diffuse, spheroidal appearance and pressure-supported kinematics to the effect of tidal stirring, rather these structural properties were established before infall.Finally, an emerging feature of the ultrafaint dwarfs is that some of them appear to be associated with other classic dSphs such as Sagittarius or Fornax. One example is the very recently discovered Segue 2 [110], where the kinematics support the association with the Sagittarius stream and with other similarly faint dwarfs, Bootes II and Coma (for Segue 1 recent work does not support the same association; see Geha et al. [111]). It is then natural to postulate that many if not all of these ultrafaint dwarfs are indeed satellites of satellites, the luminous counterparts of subhalos of subhalos seen in the latest generation of cosmological simulations resolving scales of tens of parsecs [108]. However, establishing such a link will require further studies since current cosmological simulations capable of resolving satellites of satellites do not include the baryons yet. If they were accreted as members of subgroups, the ultrafaint dwarfs might have undergone tidal stirring, and perhaps even ram pressure stripping, by a larger parent dwarf before falling into the Milky Way or M31 halo [24, 68]. The first cosmological, hydrodynamical simulations of the formation of low mass galaxies (with masses comparable with the likely progenitors of Sagittarius or Fornax) are under way as we write [89]. They will be the first step to study the nature of satellites of dwarf galaxies and assess how plausible the idea that many of the ultrafaint dwarfs are satellites of satellites.


## 9. Towards a Coherent Picture: Two Populations of dSphs Produced by the Combined Action of Tides, Ram Pressure, and the Cosmic Ionizing Background

According to the scenario that we presented in this paper, a coherent paper is emerging on the role of environment in shaping the nature of dwarf spheroidal galaxies. In particular, we posited two main formation paths for dwarf spheroidals: one for the classic dSphs and one for the ultrafaint dwarfs. Classic dwarf spheroidals live in tidally truncated halos with present-day masses of 107-108M⨀, which were typically a factor of 10, more massive, 108-109M⨀, before infall into the halos of the Milky Way and M31. They were thus born in halo potential wells too deep for suppression of gas accretion and/or photoevaporation to play a major role in determining their final properties. Instead, we argue that their current properties, including their baryonic content and mass-to-light ratio, were determined mostly by the effect of ram pressure and tides after infall into the potential of the primary galaxies, with the cosmic UV background still playing some role in the thermodynamics of the gas and in regulating star-formation both before and after infall. For classic dSphs two main outcomes are then possible depending on when they were accreted by the primary halo. At z>1, when the cosmic ionizing UV background is more than an order of magnitude higher than today, infalling dwarfs underwent complete stripping of their gas after one or two orbits and rapid truncation of star formation. This early infall mode explains an object like Draco, with a star formation history truncated about 10 billion years ago and a very high mass-to-light ratio. At z<1, the weaker UV background implies colder and more tightly bound gas in the infalling dwarfs; stripping is thus less efficient and does not lead to complete gas removal. Instead, the remaining gas is consumed in bursts of star-formation at pericenter passages due to bar-driven inflows and tidal compression. This late infall mode explains dSphs like Fornax, with an extended star formation history and moderate mass-to-light ratio. For both early and late “infallers”, we argue that they had a disky, rotating stellar component before infall, as in most present-day dIrrs, that was later turned into a pressure-supported spheroidal by tidally induced instabilities and tidal heating, a transformation mechanism that we dubbed tidal stirring. On the other hand, for ultrafaint dwarfs the formation path is governed by the effect of reionization, as expected based on their much lower mass scale, which would place them in halos with masses <107M⨀ even prior to prolonged tidal mass loss within the primary halo. They were likely born as spheroidal, pressure-supported objects before reionization, and lost most of their baryons due to photoevaporation thereafter (“reionization fossils”). In light of this scenario it is then clear how to interpret the the anticorrelation between luminosity and M/L [52], which extends all the way from Fornax to Segue 1, one of the faintest newly discovered dwarfs. This is the result of ram pressure and tidal stripping combined with the UV background at the bright/high mass end (σ>6 km/s, corresponding to an initial Vpeak>20 km/s before infall), and the product of photoevaporation by the UV background at the faint/low mass end (σ<6 km/s, corresponding to an initial Vpeak<15–20 km/s before infall). It remains to demonstrate quantitatively that the efficiency of these various mechanisms for the removal of the baryons in dwarfs increases with decreasing mass in the way implied by the observed correlation.Finally, Kravtsov et al. [24] have noted how the radial distribution of present-day dSph satellites of the MW and M31 can be used to constrain different scenarios for their origin. Dwarf spheroidals appear to be more clustered towards the center of the primary compared to the average subhalos, hence they have a steeper than average radial distribution profile. By comparing the distribution of various subsets of the substructure population of MW-sized halos in cosmological simulations with the one observed for dSphs, they were able to exclude, for example, models in which dSphs are hosted by the most massive substructures [36], while they found acceptable models in which dSphs are some of the most massive substructures prior to infall (this being consistent with the assumption behind all our works, namely, that they lost a significant fraction of their mass since they were accreted). Strigari et al. [44] reached analogous conclusions based on the analysis of the mass function of the most massive substructures. The question is as follows would tidal stirring be consistent with the observed radial distribution of dSphs? This will have to be investigated dirctly in cosmological simulations with hydrodynamics and star formation and with enough resolution to study the satellites' population. New simulations obtain a radial distribution profile of luminous subhalos that is comparable to that of observed dSphs [112] but they do not have enough resolution to explore the morphologies of luminous satellites yet, nor can they reliably model hydrodynamical mechanisms such as ram-pressure stripping. However, for the time being, there is no expected inconsistency. Indeed the assumption that the dark-matter-dominated dSphs had to be accreted at z>1, for the morphological transformation to be effective [41] naturally implies that they were accreted on fairly tight orbits (high orbital energy, short orbital times); this automatically implies a radial distribution profile steeper than that of the overall satellites’ population.


## 10. Caveats, Alternatives, and Future Prospects: Thick Disks, Infalling Subgroups, and Dark Matter Cores

The tidal stirring simulations carried out so far have always assumed an initial configuration in which the disky progenitor is constructed using an equilibrium model with a relatively thin disk of gas and stars. In reality the stellar disks of dwarfs withVc<40 km/s are expected to be rather thick as the gas that formed the disk in low mass halos reached centrifugal equilibrium with a fairly high scale height at the mean temperature of 1.5–3×104 K expected in the presence of the cosmic ionizing background at z>1 [77]. Thermal pressure, as opposed to rotation, would be crucial to explain the initial equilibrium structure of dwarfs embedded halos with Vc<20 km/s that likely hosted the progenitors of ultrafaint dwarfs. At some level it may also have affected the initial conditions of massive systems that produced the classic dSphs, and thus should be investigated further with models capable of capturing the multiphase structure of the ISM. A more diffuse, hotter stellar component argues in favor of a stronger effect of tides, but dynamical instabilities such as the bar and buckling instabilities invoked in tidal stirring are physically associated to an initially cold, rotating stellar configuration. Gas stripping by ram pressure should instead be enhanced in an initially hotter, more diffuse stellar system because of the reduced gravitational restoring force of the gas. We are currently investigating the tidal stirring and ram pressure of a realistic gas-rich dwarf with a turbulent, multiphase interstellar medium formed self-consistently in a cosmological simulation (Callegari, Mayer et al., in preparation).Recently, an alternative model has been proposed according to which some of the classic dSphs did not fall into the Milky Way halo as individual satellites but rather joined the system as part of a subgroup centered around the Large Magellanic Cloud [68]. That some satellites are brought inside of the primary halo as part of subgroups is indeed found in cosmological simulations [24, 113]. The model is not necessarily in contrast with the general tidal stirring scenario since the dwarf might have been tidally perturbed significantly by the LMC, which is 1-2 orders of magnitude more massive than even the brightest among dSphs (Fornax), and then stirred even more by the Milky Way as the subgroup was broken up by the tides of the latter soon after infall. This model would explain the possible alignment of some of the dSphs with the orbits of the Magellanic Clouds. It would also imply that a large fraction, if not half of the luminous dSphs, came in as satellites of the LMC. This would be naturally explained by how the cooling time scales with halo mass. Gas removed by the cosmic ionizing background or by tidal/ram pressure stripping as the dwarfs were part of the LMC system would have been reaccreted much more easily by the subhalos relative to the case in which they would be part of a larger halo such as that of the Milky Way. In fact, assuming that such gas would quickly thermalize with the ambient gas temperature, reaching thus the virial temperature of the primary halo, the cooling time would be much shorter (tcool≪Thubble) at the virial temperature of the LMC halo, ~105 K. However, in this model it is still unclear why dSphs have two main modes of star formation history (truncated or bursty and extended) that do not appear to be linked with their being part of the putative LMC subgroup. That being said, the potential wells of the dSphs halos might be sufficiently deep to reaccrete gas while they are still embedded in groups with the virial masses as those of the LMC halo, possibly undergoing an extended star formation history. It will be interesting to assess if other intermediate mass galaxies in the Local Group, such as M33, massive enough to be a primary of a subgroup, have dSphs, surviving or already disrupted into streams, associated to them. Future surveys of the M31 system will shed light on this possibility.Previous work has shown that a cuspy dark matter halo fitted by an NFW or Moore profile might develop a core as a result of a strong mass outflow such as that caused by supernovae winds during a burst of star formation [100]. More recently, the first high-resolution cosmological simulations of dwarf galaxy formation have shown that this mechanism may indeed be efficient at high redshift in the low mass progenitors of present-day gas-rich dwarfs, producing a galaxy with a kiloparsec-scale core at z=0 whose slowly rising rotation curve matches those of typical late-type dwarfs (Governato, Brook, Mayer et al., in prep.). A clumpy, turbulent interstellar medium may also contribute to core formation via exchange of energy and angular momentum with the surrounding dark matter halo [114]. It is thus possible that the progenitors of Local Group dSphs had a cored halo when they accreted onto the Milky Way and M31. The scenario for baryonic stripping presented in this review is mostly based on dwarf galaxy models with cuspy (NFW) dark matter halos. Our conclusions regarding the crucial effect of the environment for dSphs would be even stronger if their progenitors had cores. Indeed, the various modes of ram-pressure stripping discussed earlier are all enhanced if the gravitational restoring force is lower in the inner region of the dwarf, as expected in a constant density core. Tidal shocks will also be enhanced because the response of the system will be more impulsive with a central core, rendering the instabilities and the resulting morphological transformation more efficient. Indeed this was observed in Mayer et al. [18], where NFW halos were first introduced in dwarf galaxy models, as opposed to Mayer et al. [13, 14], where truncated isothermal halos with a small core of a few hundred parsecs were used. Other mechanisms that can enhance considerably the intensity of tidal shocks are disk shocking (see pages 21-22 and [73]) and resonances. D'Onghia et al. (2009b) have recently shown that disky satellites that plunge close to the disk of a more massive companion can undergo a resonant interaction between their rotational motion and their orbital motion which can heat the stars into a spheroid, along with stripping a large fraction of them, after only one close pericentric passage. This happens when the spin angular frequency of the disk of the dwarf and the angular frequency of its orbit are commensurate, and the spin angular momentum and orbital angular momentum are nearly aligned (that is, in a nearly prograde encounter). This mechanism could be an important extension of tidal stirring, perhaps crucial to explain dSphs orbiting far from the primary, such as Tucana and Cetus in the LG. Ongoing studies aimed at characterizing in detail the stellar component of these isolated dSphs, including their star formation history, will soon provide useful constraints on these new ideas (e.g., [115]; see also http://www.iac.es/project/LCID). Such individual, close encounters may have been more common when the primary halo was still in the process of assembling from subgroups and their subhalos were interacting with much larger companions, the size of the LMC or so. Some of such encounters may have also resulted into mergers between dwarfs since the typical velocity dispersions in subgroups should have been quite low. Whether this could be another channel of early dSphs formation is currently under investigation (Klimentowski et al., in preparation). While all these different tidal mechanisms relying on the idea of preprocessing, the morphology of the dwarf satellite population before they are accreted by the primary may play a role at some level; they need to be consistent with the morphology-density relation, a crucial constraint that tidal stirring can naturally satisfy.As our understanding of dwarf galaxy formation from cosmological initial conditions improves, interaction simulations will have to be revisited to better calibrate the quantitative effects of the various mechanisms discussed in this review. While tidal stirring may be only one part of the overall picture of dSphs formation and evolution, the new studies just recalled to reinforce the idea that tides, in various forms and at different stages of the evolution of satellites, played a key role in shaping dSphs as they are today. “Nurture” rather than “nature” is thus the most likely explanation of the origin of the classic dSphs.



---

*Source: 278434-2010-01-26.xml*