Issue 
A&A
Volume 602, June 2017



Article Number  A17  
Number of page(s)  16  
Section  Stellar structure and evolution  
DOI  https://doi.org/10.1051/00046361/201630149  
Published online  24 May 2017 
Massive star formation by accretion
II. Rotation: how to circumvent the angular momentum barrier?
^{1} Observatoire de Genève, Université de Genève, chemin des Maillettes 51, 1290 Sauverny, Switzerland
email: lionel.haemmerle@unige.ch
^{2} Institut für Theoretische Astrophysik, Zentrum für Astronomie der Universität Heidelberg, AlbertUeberleStr. 2, 69120 Heidelberg, Germany
^{3} Interdisziplinäres Zentrum für wissenschaftliches Rechnen der Universität Heidelberg, Im Neuenheimer Feld 205, 69120 Heidelberg, Germany
^{4} IRAP, UMR 5277 CNRS, 14 Av. É. Belin, 31400 Toulouse, France
Received: 28 November 2016
Accepted: 2 March 2017
Context. Rotation plays a key role in the starformation process, from prestellar cores to premainsequence (PMS) objects. Understanding the formation of massive stars requires taking into account the accretion of angular momentum during their PMS phase.
Aims. We study the PMS evolution of objects destined to become massive stars by accretion, focusing on the links between the physical conditions of the environment and the rotational properties of young stars. In particular, we look at the physical conditions that allow the production of massive stars by accretion.
Methods. We present PMS models computed with a new version of the Geneva Stellar Evolution code selfconsistently including accretion and rotation according to various accretion scenarios for mass and angular momentum. We describe the internal distribution of angular momentum in PMS stars accreting at high rates and we show how the various physical conditions impact their internal structures, evolutionary tracks, and rotation velocities during the PMS and the early main sequence.
Results. We find that the smooth angular momentum accretion considered in previous studies leads to an angular momentum barrier and does not allow the formation of massive stars by accretion. A braking mechanism is needed in order to circumvent this angular momentum barrier. This mechanism has to be efficient enough to remove more than two thirds of the angular momentum from the inner accretion disc. Due to the weak efficiency of angular momentum transport by shear instability and meridional circulation during the accretion phase, the internal rotation profiles of accreting stars reflect essentially the angular momentum accretion history. As a consequence, careful choice of the angular momentum accretion history allows circumvention of any limitation in mass and velocity, and production of stars of any mass and velocity compatible with structure equations.
Key words: stars: formation / stars: evolution / accretion, accretion disks / stars: rotation / stars: massive / stars: premain sequence
© ESO, 2017
1. Introduction
Star formation requires mechanisms that extract angular momentum from collapsing cores. If angular momentum was locally conserved during the collapse, initial turbulent motions would lead to high rotation velocities as contraction proceeds, exceeding the breakup velocity and preventing the collapse towards stellar densities (Spitzer 1978; Bodenheimer 1995; Maeder 2009). Observed rotation velocities of T Tauri stars reveal angular momentum losses during the premain sequence (PMS) evolution efficient enough to maintain the rotation period of contracting stars to a constant value despite a decrease in the moment of inertia by several orders of magnitude (Bouvier et al. 1997). This fact is thought to result from the action of the convective dynamo of lowmass stars that produces a magnetic field and couples contracting stars to their accretion discs at large distances (Koenigl 1991).
Rotating models of PMS lowmass stars have been published by several authors (e.g. Pinsonneault et al. 1989, 1990; Bouvier et al. 1997; Eggenberger et al. 2010, 2012; Amard et al. 2016). The PMS evolution of lowmass stars is expected to proceed essentially through a canonical constant mass contraction due to their long KelvinHelmholtz (KH) time (Hayashi 1961; Larson 1969; Stahler 1983), meaning that accretion can be neglected. In contrast, PMS evolution of intermediate and highmass stars is dominated by accretion ((Bernasconi & Maeder 1996; Norberg & Maeder 2000); Behrend & Maeder 2001), at rates as high as 10^{3}M_{⊙} yr^{1} (Wolfire & Cassinelli 1987). But models including accretion and rotation simultaneously and selfconsistently are still lacking.
PMS models at high accretion rates have been computed by different authors, without the effects of rotation (Omukai & Palla 2001, 2003; Yorke & Bodenheimer 2008; Hosokawa & Omukai 2009; Hosokawa et al. 2010, 2013). According to these models, rapid accretion can significantly modify the stellar structure and the evolutionary track compared to the lowrate case relevant for lowmass star formation, in particular by enhancing the swelling experienced by accreting PMS stars, leading to radii larger than 100 R_{⊙}. This swelling corresponds to the increase in the stellar radius produced by the internal luminosity wave (first described by Larson 1972), i.e. the internal redistribution of entropy when the opacity in central regions decreases abruptly. But the sensitivity of the swelling on the physical conditions makes PMS evolution with rapid accretion an open issue. In Haemmerlé et al. (2016, hereafter Paper I, we showed that with accretion through a disc, the swelling can be significantly inhibited by choosing initial conditions with a high entropy content. We expect the rotational properties of PMS stars to differ significantly depending on the details of these evolutionary features. Including rotation in accreting models could thus give useful constraints on the formation scenario of massive stars.
Recently, Lee & Yoon (2016) studied the effect of rotation on the evolution of Population III stars that accrete at rates as high as 4 × 10^{3}M_{⊙} yr^{1}. Indeed, at zero metallicity, the absence of dust and heavy elements makes the prestellar clouds hotter, the Jeans masses larger, and the accretion rates higher. At such high rates, the star approaches the Eddington limit during the swelling (Omukai & Palla 2001, 2003). Moreover, with fast rotation, the centrifugal force lowers the effective Eddington limit; the socalled ΩΓlimit (Maeder & Meynet 2000). Lee & Yoon (2016) obtained that the ΩΓlimit is reached at masses of 20 to 40 M_{⊙}, preventing further accretion. However, rotation in their models was not treated simultaneously with stellar evolution, but postprocessed from nonrotating models computed with the MESA code (Paxton et al. 2011, 2013, 2015). This procedure did not allow for inclusion of differential rotation, and the authors assumed solidbody rotation. Moreover, they considered a unique class of angular momentum accretion histories, taking in each model a constant fraction of the Keplerian angular momentum. Interestingly, we notice that in their models, at 10^{3}M_{⊙} yr^{1} the preMS swelling leads to radii lower than 20 R_{⊙}, which supports our result in Paper I that a high initial entropy content can drastically inhibit the swelling.
In Haemmerlé et al. (2013), we presented models including accretion and rotation simultaneously. However, these models were computed with an old version of the Geneva code, that contained an inconsistency in case of accretion. The treatment of accretion in the Geneva code has recently been improved (Haemmerlé 2014). We described in Paper I the effects of these improvements in the nonrotating case. The present paper is devoted to the case with both accretion and rotation simultaneously. These improvements allow us to present here the first PMS models for the formation of massive stars that include accretion and rotation simultaneously and selfconsistently. In Sect. 2, we describe the treatment of rotation in the code and the physical conditions assumed in our models. Section 3 is devoted to the effect the various physical conditions have on PMS evolution. In Sect. 4, we present a birthline computed with the effect of rotation and we look at the impact of PMS evolution with accretion of angular momentum on the MS evolution. We discuss our results in Sect. 5 and summarise our conclusions in Sect. 6.
2. Rotation in the Geneva code with accretion
2.1. Improvements in the code
A full description of the treatment of accretion in the Geneva Stellar Evolution code has already been given in Paper I in the nonrotating case. We described the recent improvements to the code and how they modify the results compared to the versions used in Bernasconi & Maeder (1996), Norberg & Maeder (2000), Behrend & Maeder (2001) and Haemmerlé et al. (2013). A detailed description of the treatment of rotation without accretion in the code is given in Eggenberger et al. (2008). In the present section, we describe how the treatment of rotation with accretion is improved in the new version of the code A full description of the simultaneous treatment of accretion and rotation in the new version of the code is also available in Haemmerlé (2014).
The new improvements in the code are related to the time derivatives and the resulting time variation of the physical quantities. Among the four equations of structure, the only one that refers to time is the equation of energy conservation, which reads (1)where M_{r} is the mass enclosed in a shell of radius r, L_{r} the luminosity at r, ϵ_{n} the energy generation rate by nuclear reactions, T the temperature, s the specific entropy and t the time. Thus it is the equation that makes the star evolve. As described in detail in Paper I, in the new version of the code, we removed an inconsistency in this equation that leads to artificial loss of entropy and to artificially low radii during the PMS swelling phase. However, when we add rotation, we have to solve, in addition to the usual equations of stellar structure, the equation of angular momentum transport. In the Geneva code, rotation is treated with the assumption of shellular rotation (Meynet & Maeder 1997): differential rotation is allowed in the radial direction, but we force the angular velocity to be uniform on each isobar. The justification of this assumption is that horizontal turbulence that is produced by differential rotation is efficient enough to maintain each isobar in solidbody rotation (Zahn 1992). In addition, each convective region is also assumed to rotate as a solid body. In radiative regions, two types of rotational instabilities are included: diffusion by shear and advection by meridional currents. The equation of angular momentum transport reads (2)where Ω is the angular velocity, U(r) the amplitude of the radial component of the meridional velocity, and D(r) the diffusion coefficient for shear instability (using the prescription of Maeder 1997). We note that no magnetic field is taken into account. In particular, no TaylerSpruit dynamo is included. However, we discuss the effect of an internal magnetic coupling in a semianalytical way in Sect. 5.4.
As Eq. (1), Eq. (2) refers to time through the Lagrangian derivative (of the angular momentum in this case) (3)The spatial coordinate used in the Geneva code is not, however, the Lagrangian coordinate M_{r}, but the relative mass coordinate (4)In the presence of accretion, μ is not a Lagrangian coordinate since M increases with time. With this coordinate, Eq. (2) becomes Equation (6) contains an additional term compared to Eq. (2), which is proportional to the accretion rate and the internal gradient of angular momentum. Since, in general, the angular momentum increases outwards and Ṁ> 0 during accretion, this additional term is negative. In the previous version of the code, the effect of this additional term was neglected, leading to artificial loss of angular momentum. Indeed, if we neglect this negative term, the term in d(r^{2}Ω)/dt has to be smaller. The effects of these improvements on the models are illustrated in Appendix A.
2.2. Angular momentum accretion rate
When we add rotation in the context of accretion, we also have to specify, in addition to the mass accretion rate, the angular momentum accretion rate (7)where j_{accr} is the specific angular momentum of the material that is accreted.
The procedure applied in order to accrete angular momentum in the Geneva code is the following. When we accrete mass during a timestep dt, we add a new layer in the outer boundary of the stellar interior, defined as the region where M_{r}/M< fit_{M} for a given value of fit_{M} (typically fit_{M} = 0.999). In the envelope (M_{r}/M> fit_{M}), several simplifying assumptions are made, for reasons of numerical stability. In addition to assuming that dL_{r}/ dM_{r} = 0, we assume in the rotating case that the envelope rotates as a solid body, with the same angular velocity as the external layer of the interior. The new layer added between the interior and the envelope is defined as having exactly the mass accreted during dt, that is, dM = Ṁ dt. Once this layer has been added, we have to define its physical properties. The choice of the thermal properties of this new layer has already been described in Paper I, and corresponds to the assumption of cold disc accretion. In the rotating case, we also have to specify the angular velocity Ω_{accr} of this new layer, that we choose to be (8)where r_{fitm} is the radius corresponding to M_{r}/M = fit_{M}. The factor 2/3 in Eq. (8)reflects the fact that the material is distributed over a spherical shell.
In the present work, we use various prescriptions for . The first is the smooth angular momentum accretion (“smoothJ” hereafter), which states that the angular velocity of the material that is accreted is the same as that of the stellar surface before the material is added. This prescription was used in Haemmerlé et al. (2013). We note that in this case, the only free parameter for rotation is the rotation velocity of the initial model. In the second case considered here, we aim to fix a constant value of j_{accr} = dJ/ dM, that is, the specific angular momentum in the accreted material. This gives an angular momentum accretion rate that is proportional to the mass accretion rate from Eq. (7). However, the accretion of angular momentum in the Geneva code cannot be controlled as freely as the accretion of mass in the cases where angular momentum transport is significant in the external layers of the star, for instance when the external layers are convective, which implies instantaneous angular momentum redistribution. In Sect. 4, we use a slightly different prescription, with j_{accr} ∝ M^{0.8}. Finally, in Appendix B, we discuss the case of angular momentum accretion according to a constant fraction of the Keplerian value.
The physical justifications of these angular momentum accretion laws are related to the complex mechanisms that govern the inner part of accretion discs, such as magnetic fields, viscosity, or gravitational instability. The role of these mechanisms in regulating the accretion of angular momentum is still far from being fully understood. Observations of discs around massive young stellar objects (MYSOs) are in good agreement with Keplerian rotation profiles (Cesaroni et al. 2005; Kraus et al. 2010; Keto & Zhang 2010; Ilee et al. 2016), but the inner part of these discs are out of the reach of current observations. At the stellar surface, the Keplerian velocity corresponds to the critical limit beyond which accretion from the disc onto the star cannot occur. The critical velocity is defined as the rotation velocity at the stellar surface at which the centrifugal force cancels gravity (i.e. ) and corresponds to the upper limit compatible with hydrostatic equilibrium. Thus a braking mechanism is expected in the inner region of the discs, probably related to the magnetic field (Pudritz et al. 2007; Hennebelle & Ciardi 2009; Joos et al. 2012; Seifried et al. 2013, 2015), the disc viscosity (Vorobyov & Basu 2009; Stacy et al. 2011), or the gravitational torques (Jappsen & Klessen 2004; Vorobyov & Basu 2007). The magnetic field of massive MS stars is still an uncertain issue given the absence of a surface convective dynamo and the small number of magnetic fields detected at the surface of observed massive stars (see e.g. Grunhut et al. 2017). The common existence of outflow jets around MYSOs accreting at high rates (Arce et al. 2007; Dougados 2009; Reiter & Smith 2013, 2014; Reiter et al. 2015b,a) indicates that magnetic fields play a significant role in the accretion process for massive star formation (Guzmán et al. 2010; Whelan et al. 2010; Ellerbroek et al. 2014). Such outflow jets are not necessarily due to stellar magnetic fields, and could result from magnetised disc winds (Pudritz & Banerjee 2005; Pudritz et al. 2007) or a superposition of aligned outflows from many lowmass stars that usually form alongside massive stars (Peters et al. 2014). But, whatever the mechanism that launches the jets, the fraction of angular momentum carried away can eventually represent a significant fraction of the Keplerian value (Bodenheimer 1995; Pudritz et al. 2009). Additionally, PMS objects that are destined to become massive stars by accretion have a large convective envelope during their early accretion phase (see e.g. Paper I), which could potentially produce a magnetic field. The geometry of the accretion flow close to the stellar surface depends sensitively on the geometry of the magnetic field, which is poorly constrained (Pudritz et al. 2007; Romanova & Owocki 2015). Whether the intersections between the field lines and the stellar surface are concentrated near the poles or distributed isotropically, the amount of angular momentum that is accreted will be significantly modified. The exact determination of the angular momentum accretion history for realistic geometries of the magnetosphere goes far beyond the scope of the present work, and here we only consider arbitrary assumptions in order to explore the various possible scenarios. The smoothJ accretion corresponds to the case where the rotation of the star is imposed to the inner parts of the accretion disc, but assuming that this inner region does not influence the rotation of the star. As we will see, this accretion law leads the rotation of the star to become critical when, typically, masses of approximately 8 M_{⊙} are reached. This clearly indicates that a coupling between the star and the inner disc must operate preventing the star from reaching the critical limit. The constantj_{accr} accretion corresponds to the case where the accreted material is not influenced by the rotation velocity of the stellar surface, and where any braking occurs upstream in the accretion flow.
3. Impact of the physical conditions on PMS evolution with accretion and rotation
3.1. SmoothJ accretion: model at low massaccretion rate
We first describe a test model computed with the new version of the code at the low constant massaccretion rate of (9)assuming smoothJ accretion, as in Haemmerlé et al. (2013). Initial conditions are given by (10)with solar composition^{1}. This initial model has a radius of 6.06 R_{⊙} and is fully convective. Since solidbody rotation is assumed in convective regions, a unique value of the angular velocity defines the whole rotational inputs, here (11)Such velocity is extremely low for a PMS star of 0.7 M_{⊙} (smaller than 1% of the critical velocity, Eq. (11)). The reason for this choice is presented below. For the moment, we only notice that the models have been computed for almost the whole PMS phase. For the considered massaccretion rate, this corresponds to the low and intermediatemass range: M ≲ 8M_{⊙}.
Fig. 1 Evolution of the internal structure, the angular momentum accretion rate, and the equatorial surface velocity of the testmodel at low massaccretion rate described in Sect. 3.1, as a function of the increasing stellar mass, which is a timecoordinate in the case of accretion. Upper panel: radius (blue curve) and the internal structure, with convective zones in dark grey and radiative zones in light grey. The dark grey dotted curves are isomass of M_{r} = 1, 2, 3,..., M_{⊙}. Second panel: angular momentum accretion rate in logarithm of . Third panel: surface velocity (at the equator) and the fourth panel shows the ratio of the surface velocity to the critical velocity. (The critical limit is indicated by the horizontal grey dotted line.) 
The evolution of the internal structure of this model is shown in the upper panel of Fig. 1. At such a low rotation velocity, the effect of rotation on the evolutionary tracks (not shown here) and on the internal structure is negligible, as with the original version of the code (see Haemmerlé et al. 2013). A detailed description of the evolution of the internal structure for such a model can be found in Paper I; here we summarise the main features. The evolution starts with a fully convective structure. The internal temperature is initially too low for nuclear burning, and the star takes its energy from gravitational contraction. The radius decreases and the central temperature grows, until it exceeds ~ 10^{6} K (at M ≃ 1M_{⊙}). Following this, Dburning starts in the centre, the temperature stops growing, and the radius increases (T_{c} ∝ M/R). When D is exhausted, the star has to contract again, the radius decreases, and the central temperature grows again. As a result, the opacity decreases, and at M = 2.4M_{⊙}, a radiative core appears and grows in mass. The high luminosity emerging from this hot radiative core is absorbed by the cold convective envelope, which expands (luminosity wave, Larson 1972; Hosokawa et al. 2010); the star experiences a rapid swelling, that leads in this case to a maximum radius of 10.4 R_{⊙}. At that point, the convective envelope has disappeared and the fully radiative star goes through a KH contraction.
The second panel of Fig. 1 shows the evolution of (Eq. (7)), that is, the angular momentum accretion rate given by the assumption of smoothJ accretion. The value of j_{accr} increases as the stellar mass grows, by two orders of magnitude between 0.7 and 6 M_{⊙}. The surface velocity at the equator (third panel) increases by almost three orders of magnitude in the same interval. We notice that the increase becomes particularly strong for M> 5M_{⊙}, which corresponds to the phase of postswelling KH contraction (upper panel), where the external layers contract rapidly (see the isomass of 5 M_{⊙}).
The lower panel of Fig. 1 shows the evolution of the ratio v_{surf}/v_{crit}. The model starts with a surface velocity smaller than 1% of the critical value, following the assumptions described in Eq. (11). Then, due to the increase of the stellar mass by one order of magnitude during the PMS, the critical velocity increases slightly. However, since the surface velocity increases by three orders of magnitude during the same phase, the ratio v_{surf}/v_{crit} increases by more than two orders of magnitude. As a consequence, in this model, the stellar surface reaches the critical velocity at a mass of (12)The critical velocity is the maximum value of the surface rotation velocity for a star in hydrostatic equilibrium; if the surface velocity increases above this value, the centrifugal force dominates over gravity, accretion stops, and the star begins to lose mass. As a consequence, masses higher than this M_{max} cannot be reached in this scenario, that is, the star cannot enter the range of massive stars. In the present models, we did not include any massloss: we simply stopped the computation when v_{surf} = v_{crit}.
Fig. 2 Internal rotation profiles of the model at low massaccretion rate described in Sect. 3.1 for evolutionary stages M = 2, 4, and 6 M_{⊙}, as a function of the Lagrangian coordinate M_{r}. The upper panel shows the profiles of the specific angular momentum while the lower panel shows the angular velocity Ω. 
In order to understand the evolution of the surface rotation velocity, we look at the internal rotation profiles along the evolution, when the model reaches stellar masses of 2, 4, and 6 M_{⊙} (Fig. 2). As is visible in the upper panel of Fig. 1, the star is still fully convective at M = 2M_{⊙}. At 4 M_{⊙}, the radiative core has grown to M_{r} = 3 M_{⊙}, so that the convective envelope still covers 25% of the stellar mass. At 6 M_{⊙}, the star is fully radiative. The upper panel of Fig. 2 shows the profiles of the specific angular momentum on each shell of radius r, explicitly: (13)where v_{eq}(r) is the equatorial velocity of the shell of radius r. Except in convective regions, the jprofiles match one another. This means that angular momentum is locally conserved in radiative regions, that is, angular momentum transport by shears and meridional circulation is negligible in the short timescale of the accretion phase. The profiles at 2 and 4 M_{⊙} differ due to the assumption of solidbody rotation in convective regions, implying instantaneous angular momentum redistribution in cases of nonhomologous contraction. The profiles at 4 and 6 M_{⊙} differ only slightly in the layers with 3 M_{⊙}<M_{r}< 4 M_{⊙}, corresponding to the convective envelope in the 4 M_{⊙} profile. Given the jprofiles, the Ωprofiles (Fig. 2) depend solely on the relative contraction of each layer. Solid rotation in convective zones is reflected in a flat Ωprofile at M = 2 M_{⊙}, as well as in the layers with M_{r}> 3 M_{⊙} of the profile at M = 4 M_{⊙}. In radiative regions, the rapid contraction of the external layers (Fig. 1, upper panel) leads to Ωprofiles that increase outwards (). In particular, during the postswelling contraction, the external layers contract in a very short time (isomass of 5 M_{⊙} on the upper panel of Fig. 1), leading to high rotation velocities (notice the logarithmic scale). This is the reason why the surface velocity reaches the critical value during this stage.
3.2. Varying the initial rotation velocity
As mentioned in Sect. 2, in the case of smoothJ accretion, the value of the initial rotation velocity fixes the whole rotational history of the star. In Sect. 3.1, we showed that starting from a low rotation velocity, the critical limit is reached before the star enters the range of massive stars. Now, we try to decrease the initial rotation velocity even more, by one order of magnitude, and we consider a model with (14)Except for the rotation velocity, we consider the same initial model as in Sect. 3.1 (Eq. (10)), and we compute a birthline with the new version of the code, again at 10^{5}M_{⊙} yr^{1}.
The evolution of the surface rotation velocity of this model is shown in Fig. 3. As for the faster rotator described in Sect. 3.1, the surface velocity increases by several orders of magnitude along the intermediatemass range. Again, the increase is particularly strong during the postswelling contraction (M ≳ 5M_{⊙}). In this case, due to the low initial velocity, the stellar surface reaches the critical velocity at a slightly higher mass than for the faster rotators described in Sect. 3.1. Here the maximum mass that can be accreted is (15)Although this value is higher than that of the previous case, the difference remains relatively small. Indeed, we see that when we decrease Ω_{ini} by one order of magnitude, we increase M_{max} by 17% only. As a consequence, even with this lower initial velocity, the star cannot enter the highmass range.
3.3. Varying the mass accretion rate
We now consider various accretion rates in order to see how the choice of the accretion history can affect the internal structure of the star and its final mass. The accretion rate used in Sect. 3.1 is lower than what is expected for massive star formation, and we consider, here, more appropriate rates, such as a constant rate of 10^{3}M_{⊙} yr^{1}, and the ChurchwellHenning (CH) accretion law.
The CH law (Behrend & Maeder 2001) has been described in detail in Paper I, where we have shown that it reproduces well the upper envelope of Herbig Ae/Be stars on the HertzsprungRussell (HR) diagram. This law depends on a parameter f, which reflects the fraction of the mass from the accretion flow that is effectively accreted by the star, the rest being ejected through bipolar outflows. As shown in Paper I, the best fit for intermediate and highmass stars is obtained with f = 1/11, and thus we use this value in the present section. We recall here that this rate is time dependent, increasing with the evolution, from ~ 10^{5}M_{⊙} yr^{1} in the low and intermediatemass range to ~ 10^{3}M_{⊙} yr^{1} in the highmass range.
Numerical convergence is difficult for lowmass models that accrete at rates as high as 10^{3}M_{⊙} yr^{1}. Thus we started the computation of the model with constant high rate at (16)This initial model has a radius of 20.5 R_{⊙} and is fully convective. In the case of CH accretion, the early accretion rate is still low and we use the same initial model as in the previous sections (Eq. (10)). In both cases, we consider Ω_{ini} = 10^{8} s^{1}.
Fig. 4 As in Fig. 1 (without v_{surf}), for the model with Ṁ = 10^{3}M_{⊙} yr^{1} and Ω_{ini} = 10^{8} s^{1}, described in Sect. 3.3. The isomass corresponds to M_{r} = 2, 4, 6,..., M_{⊙}. 
Fig. 5 As in Fig. 1 (without v_{surf}), for the model with CH accretion and Ω_{ini} = 10^{8} s^{1}, described in Sect. 3.3. 
The evolution of the ratio v_{surf}/v_{crit} for these two rates is shown in Figs. 4 and 5. In both cases, the surface velocity and the specific angular momentum accreted increase monotonically, with a particularly abrupt jump during the swelling phase, when the convective envelope disappears, and the external layers of the fully radiative star contract rapidly. It leads to the critical limit, ending the accretion process at (17)for 10^{3}M_{⊙} yr^{1} and CH accretion, respectively. Notice that when the surface velocity approaches the critical limit, the effect of rotation on the stellar structure becomes significant by increasing the radius (by nearly a factor 2 in the Ṁ = 10^{3}M_{⊙} yr^{1} case). However, in the present models, such a phase is extremely shortlived, and moreover the effect concerns only the very external layers. We see here that the high constant accretion rate allows the star to enter the highmass range only marginally, while the CH rate leads to a stronger limitation than in the cases considered previously. In particular, the increase in the accretion rate by two orders of magnitude (from 10^{5} to 10^{3}M_{⊙} yr^{1}) produces an increase in M_{max} by less than a factor 2.
3.4. Varying the angular momentum accretion history
Then we try to modify the Jaccretion history by fixing a constant specific angular momentum in the accreted material (dJ/ dM = const.). However, as mentioned in Sect. 2.2, accretion of angular momentum in the Geneva code cannot be controlled as freely as the accretion of mass. Strong oscillations appear in the evolution of dJ/ dM around the desired value when angular momentum transport is significant in the external layers of the star, for instance when these layers are convective. Here we compare three different values of the specific angular momentum, j_{accr} = 1, 3, 4 × 10^{18}cm^{2} s^{1} with a fixed mass accretion rate of 10^{3}M_{⊙} yr^{1}. The initial conditions are given by Eq. (16) and Ω_{ini} = 1, 3, 6 × 10^{6} [s^{1}], respectively. The results are shown in Fig. 6. The upper panel shows the stellar structure at such a mass accretion rate in the nonrotating case, since rotation does not significantly modify the stellar structure in these cases.
Fig. 6 Varying the angular momentum accretion history, for Ṁ = 10^{3}M_{⊙} yr^{1}. Upper panel: internal structure of the nonrotating model: the upper curve is the stellar radius, the dark grey regions are convective, the light grey is radiative, and the dotted lines are iosmass of 2, 4, 6, 8,..., M_{⊙}. Second panel: three Jaccretion histories considered and the third one, specifically, shows the evolution of v_{surf}/v_{crit} for the corresponding models (the grey dotted horizontal line indicates the critical limit), and bottom panel: deformation of the star due to rotation (R_{eq} and R_{pol} are the equatorial and polar radii, respectively). 
The oscillations in j_{accr} produce oscillations in v_{surf}/v_{crit}. However, v_{surf}/v_{crit} remains clearly in the same order of magnitude throughout the evolution. In fact, v_{surf}/v_{crit} shows a slight global decrease during the PMS (M< 30 M_{⊙} at this rate); in all three cases, the initial value of v_{surf}/v_{crit} is never exceeded during the computation. In particular, despite an initial velocity as high as 75% of the critical value, the fastest rotator never approaches the critical limit during its PMS evolution. Thus in this case, no limitation in mass is encountered, and accretion can proceed freely until the zeroage main sequence (ZAMS), without fearing the centrifugal force.
Fig. 7 Internal rotation profiles of the model with Ṁ = 10^{3}M_{⊙} yr^{1} and j_{accr}≃ 4 × 10^{18}cm^{2} s^{1} (fastest rotator of Fig. 6) for M = 5, 10, 15, 20, 25, 30 M_{⊙}, as a function of the Lagrangian coordinate M_{r}. Upper panel: profiles of the specific angular moment , and second panel: profiles of the angular velocity Ω. On the bottom panel timescales for angular momentum transport by shear diffusion and meridional circulation at M = 15M_{⊙}, and compare it with the PMS timescale M_{ZAMS}/Ṁ≃ 35 000 yr. The arrows indicate the direction of the angular momentum transport by meridional currents, outwards or inwards. 
The internal rotation profiles of the fastest rotator considered here are shown in Fig. 7. As in the previous cases, the more efficient process for angular momentum transport is convection (compare the jprofiles at M = 5 and 10 M_{⊙}, and those at M = 25 and 30 M_{⊙}). But in this case, some angular momentum transport also acts in radiative regions. Indeed, by comparing the profiles at M = 15, 20, and 25 M_{⊙}, when the star is fully radiative (see the upper panel of Fig. 6), we see that j is not constant for fixed M_{r}. For instance, the value of j corresponding to the layer with M_{r} = 15M_{⊙} decreases between M = 15 and 25 M_{⊙}. This is an effect of meridional circulation, that transports angular momentum from the contracting core outwards into the external regions. This can be seen i the lower panel of Fig. 7, where we compare the timescales for angular momentum transport by shear diffusion and by meridional currents with the timescale of the PMS phase, here given by the accretion time M_{ZAMS}/Ṁ≃ 35 000 yr, where we used M_{ZAMS}= 35 M_{⊙} (see the upper panel of Fig. 6). The profiles are shown only for M = 15M_{⊙}, when the star is fully radiative. The timescale for shear diffusion, given by R^{2}/D(r), always exceeds the PMS time, by at least one order of magnitude, which means that this process is negligible on such evolutionary timescales. On the other hand, the timescale for meridional circulation, that is, the EddingtonSweet time R/U(r), becomes shorter than the PMS time in the external layers (M_{r}> 12M_{⊙}). In this region, U(r) < 0, which means that angular momentum is transported outwards. This outwards transport is responsible for the oscillations in dJ/ dM (second panel of Fig. 6). Nevertheless, this feature only concerns the surface layers, and only becomes significant for the fast rotator considered here. We note that U(r) > 0 in the inner regions (M_{r}< 4M_{⊙}), and there angular momentum is transported inwards. However, this mechanism remains inefficient here, with a characteristic timescale two orders of magnitude longer than the PMS time. Thus, the evolution of the rotational properties in radiative regions remains dominated by local angular momentum conservation, and, globally, the jprofiles reflect the Jaccretion history, as in the cases considered previously. The present Jaccretion history leads to Ωprofiles that decrease outwards, except in convective regions where it is flat (second panel of Fig. 7). In contrast to the smoothJ case, the assumption of nearly constant j_{accr} compensates for the spinning up of the fast contracting layers. Indeed, these layers are accreted at large r, and thus a constant j_{accr} implies a low Ω, according to Ω ∝ r^{2}.
Notice that, even for the fastest rotator considered here, rotation does not impact significantly the stellar structure or the evolutionary track on the HR diagram. In order to estimate the deformation (flattening) of the star due to rotation, we plotted the ratio of equatorial to polar radius on the lower panel of Fig. 6. The deformation only becomes significant (R_{eq}−R_{pol}> 10% R_{pol}) for fast rotators (v_{surf}> 50%v_{crit}), according to the Roche model. In the Roche approximation, the deformation of the star is modelled by including the centrifugal force in the hydrostatic equilibrium, but without any change in the gravitational force due to the modifications in the mass distribution induced by the deformation. This approximation gives results that are in good agreement with observed fast rotators (Peterson et al. 2006; Maeder 2009).
Fig. 8 Internal structure of the initial models described in Sect. 3.5. Upper panel: entropy profile and lower panel: Ωprofile. Entropy is computed from an arbitrary reference value s_{0} that corresponds to the high entropy CV model. In each panel, the boundary between convection and radiation in the lowentropy RC model is indicated by a dot. 
3.5. Impact of initial conditions
In Paper I, we showed that the initial stellar structure significantly impacts the PMS evolution with accretion at high rates. We found that compact radiative (RC) initial models with a low entropy content lead to a much stronger swelling than the extended convective (CV) initial models of high entropy content used above. With the RC models, the stellar radius exceeds 100 R_{⊙} during the swelling, similar to the models of Hosokawa et al. (2010). In the present section, we describe how this effect impacts the rotational history of the star.
Fig. 9 Evolution of the models described in Sect. 3.5, with Ṁ = 10^{3}M_{⊙} yr^{1} and j_{accr} ≃ 10^{18} cm^{2} s^{1}, started from the CV and the RC models (black and green lines, respectively). Upper panel: stellar radius, second panel: moment of inertia, third panel: accretion of angular momentum, and the lowest panel the ratio of the surface rotation velocity to the critical velocity. In the upper panel, the solid lines correspond to the stellar radius and the dotted lines indicate the location of the layer that encloses 90% of the actual stellar mass. In the third panel, the grey dotted line is the ideal value of j_{accr} = 10^{18} cm^{2} s^{1} while in the lowest panel, the grey dotted line indicate the critical limit and the coloured dotted lines indicate the evolution of v_{surf}/v_{crit} with the assumption of solidbody rotation (see Sect. 5.4). 
The surface properties of the CV model are given by parameters (16), and we consider Ω_{ini} = 10^{6} s^{1}, which corresponds to the slowest rotator described in Sect. 3.4, with v_{surf}/v_{crit} = 0.13. Our RC initial model is given by (18)and has a radius of 2.53 R_{⊙}. Its structure is composed of a radiative core (M_{r}< 1.53 M_{⊙}) surrounded by a convective envelope. Thus, in this case, the assumption of solidbody rotation does not apply for the whole star. We give to the RC model the same total amount of angular momentum as that of the CV model, and the rotation profile is obtained by a constantmass contraction from the CV model. The entropy profiles and the Ωprofiles of these two models are shown in Fig. 8. Since the RC model is much more compact than the CV model, the fact that we choose both to have the same amount of angular momentum leads to a faster rotation in RC than in CV. Indeed, the RC model corresponds to an initial ratio v_{surf}/v_{crit} = 0.4 instead of 0.1 for CV. Moreover, we see that the Ωprofile of the RC model is not flat, but shows differential rotation in the radiative core.
The evolution of the stellar radius, the moment of inertia, the accretion of angular momentum and the ratio of the surface velocity to the critical one are shown in Fig. 9 for models computed from CV and RD with Ṁ = 10^{3}M_{⊙} yr^{1} and j_{accr} ≃ 10^{18} cm^{2} s^{1}. While the radius of the CV model remains always below 50 R_{⊙}, that of the RC model exceeds 100 R_{⊙} during the swelling, as described in Paper I in the nonrotating case. But, counterintuitively, despite its large radius during the swelling, the RC model retains a much smaller moment of inertia than the CV model. Indeed, the initial compactness of the RC model gives it a small moment of inertia. Then, during the swelling, contraction is highly nonhomologous and the mass distribution is strongly centralised; only a small fraction of the stellar mass is contained in the extended outer layers. Most of the mass remains close to the centre, with a small moment of inertia. This is illustrated by the dotted lines on the upper panel, that show the radius enclosing 90% of the actual stellar mass; this radius remains constantly smaller for the RC model than for the CV model, even during the swelling.
As mentioned in Sect. 3.4, the constantj_{accr} assumption compensates for the variations in rotation velocity due to the swelling and the rapid contraction, because the larger the radius, the lower the velocity of the material accreted at a given j_{accr}. We see in the lower panel of Fig. 9 that the swelling does not significantly affect the ratio v_{surf}/v_{crit}; despite a few oscillations, v_{surf}/v_{crit} remains in the same order of magnitude. In fact, the values of v_{surf}/v_{crit} for the two models converge slowly as the star contracts towards the ZAMS. Despite a relatively high initial velocity (v_{surf}/v_{crit} ≃ 40%), the RC models never reach the critical limit during the PMS, and approach the ZAMS at v_{surf}/v_{crit} ≃ 10%, as in the CV case. In the constantj_{accr} case, the RC model leads to a slightly stronger decrease in v_{surf}/v_{crit} during the accretion phase, compared to the CV model. This fact does not result from the magnitude of the swelling, but simply from the fact that the initial moment of inertia is smaller in the RC case than in the CV case. Thus, producing massive stars rotating at a given surface velocity using a given angular momentum accretion history requires a higher initial ratio v_{surf}/v_{crit} in the RC case than in the CV case. This fact makes it harder to produce massive fast rotators starting from RC than starting from CV, since the initial ratio v_{surf}/v_{crit} must always be smaller than 1.
Notice that the angular momentum transport by shear diffusion and meridional circulation remains completely negligible in the RC case due to the decrease in v_{surf}/v_{crit} that leads to slow rotation. Thus, the variations in j_{accr} around the specified value are lower in the RC case than in the CV case, because the RC model is essentially radiative, with only a small convective envelope that disappears at M = 5.5M_{⊙}.
4. Birthline, PMS contraction, and MS evolution
Once a star reaches its final mass and stops accreting, its evolution proceeds according to the constant mass scenario, or with a mass that decreases with time in case of significant mass loss. For low and intermediatemass stars, accretion is expected to stop before the ZAMS (Paper I), and the further PMS phase corresponds to a classical KH contraction towards the ZAMS. In the lowmass case, the KH time exceeds the accretion time, and the timescale of the constant mass phase is expected to be much longer than that of the accretion phase. For massive stars, the ZAMS is expected to be reached before the end of accretion (Paper I). Thus, in this case, the MS phase directly follows the accretion phase. In both cases, the rapid accretion phase is followed by a much slower evolution. In the present section, we describe a birthline computed with the effect of rotation and study how it impacts the rotational properties of stars during these slow KH or MS phases. Observationally, the “birthline” is defined as the upper envelope of preMS stars on the HR diagram. In the context of a unique accretion history, it corresponds also to the evolutionary track of accreting stars. See Paper I for more details.
Fig. 10 Properties of the birthline described in Sect. 4.1. Upper panel: stellar radius (upper blue curve) and the internal structure, with convective regions in dark grey, radiative regions in light grey, and isomass as dotted curves. Second panel: accretion of specific angular momentum (in logarithm of cm^{2} s^{1}): the black dotted line is the value given by Eq. (19) and the solid blue line indicates the angular momentum effectively accreted. Third panel: angular velocity at the surface and in the centre. The lower panel shows the ratio v_{surf}/v_{crit} (lower thick solid blue line). The filled squares connected by the thin blue line indicate the values of v_{surf}/v_{crit} reached by the models at constant mass computed from the birthline once they have converged to their MS equilibrium (see Sect. 4.2). The blue dashed line shows the values of v_{surf}/v_{crit} of the same models when they reach their minimum radius corresponding to the ZAMS. We also added the value of v_{surf}/v_{crit} these models would have at the minimum radius if angular momentum was locally conserved (blue dotted line). The grey dotted horizontal line indicates the critical limit. 
4.1. Birthline
We build by accretion models for the mass range from 1 to 120 M_{⊙}. For simplicity, we consider only one single accretion scenario for mass and angular momentum. As shown in Paper I, the birthline given by the CH accretion law provides the best fit to the observations of T Tauri and Herbig Ae/Be stars. Thus we choose this law for the accretion of mass. For the accretion of angular momentum, we aim at reaching a unique value of v_{surf}/v_{crit} ≃ 0.5 on the ZAMS, which is typical for MS stars (Huang et al. 2010). We consider an accretion history given approximately by (19)Notice that the only justification of our choice of a unique accretion history for the angular momentum is the fact that the prescription of Eq. (19) allows us to reach v_{surf}/v_{crit} ≃ 0.5 on the ZAMS for all the masses considered, as shown below (Fig. 10). In particular, the exponent 0.8 in Eq. (19) is only an ad hoc value chosen to that end.
We start the computation at 0.7 M_{⊙} with initial conditions given by Eq. (10), corresponding to the CV case of Sect. 3.5, and we stop when the stellar mass reaches 120 M_{⊙}. As mentioned in Sect. 3.5, for a constant mass accretion rate of 10^{3}M_{⊙} yr^{1}, the choice of the initial model has a significant impact on the structure of PMS stars, and then on their rotational properties. However, in the case of CH accretion, this effect remains negligible, since the accretion rate is still of the order of 10^{4}M_{⊙} yr^{1} when the swelling occurs, as mentioned in Paper I. Thus we do not expect the use of RC initial conditions, instead of the CV model considered here, to significantly change the results of the present section.
The properties of the birthline we obtain with these assumptions are shown in Fig. 10. The evolution of the stellar radius and the internal structure are similar as in the cases described in Paper I and in Sect. 3. With the CH accretion law, the ZAMS is reached slightly above 20 M_{⊙}. The accreted angular momentum follows the law given by Eq. (19) relatively regularly until 50 M_{⊙}. Then, strong oscillations appear leading to a net decrease in j_{accr} for masses ~ 100M_{⊙}.
At the beginning of the evolution, the fully convective structure imposes solidbody rotation (Ω_{centre} = Ω_{surface}), but once the radiative core appears and the swelling starts, differential rotation develops due to the highly nonhomologous contraction (third panel of Fig. 10); the rapidly contracting core rotates faster than the surface, which contracts at a slower rate due to the entropy it receives from the core. At the end of the swelling, the ratio Ω_{centre}/ Ω_{surface} reaches a maximum of 7. During the KH phase that follows the swelling, the external layers can contract rapidly, and they spin up consequently. On the ZAMS (log M/M_{⊙} ≃ 1.3), however, the convective core rotates still three times faster than the surface. After that, the expansion of the central layers due to Hburning slows down the rotation of the core, while Ω_{surf} remains almost constant (j_{accr} and R are both increasing). Differential rotation is still present at the end of our computation with a core rotating two times faster than the surface. The critical limit is never reached during the evolution (lower panel of Fig. 10). Despite a slight increase in v_{surf}/v_{crit} during the accretion phase, the surface velocity remains under 50% of the critical value until the end of the computation. This behaviour simply reflects the Jaccretion history, since angular momentum transport by meridional circulation and shear turbulence also remains negligible in this model.
4.2. Evolution at constant mass
From the birthline described in Sect. 4.1, we compute the following evolution of models of various masses by switching off accretion. We include mass loss in these models, with the same treatment as in Ekström et al. (2012). The models of various masses are thus labelled by their mass at the end of the accretion phase, written here M_{ZAMS}, since mass losses are negligible during the PMS phase. We consider M_{ZAMS}=1, 5, 9, 15, 20, 40, 60 and 120 M_{⊙}. Notice, however, that stars with masses above 20 M_{⊙} reach the ZAMS before the end of their accretion phase (Sect. 4.1). Thus, strictly speaking, M_{ZAMS} is not the ZAMS mass for those models.
Only models with M_{ZAMS} ≤ 20M_{⊙} experience a PMS contraction, while for models with M_{ZAMS}> 20M_{⊙}, the accretion phase overlaps with early MS evolution. In all cases, as mentioned at the beginning of the present section, the rapid accretion phase is followed by a slower evolution, during which the angular momentum transport in radiative regions can become significant. Indeed, it is well known that meridional currents lead to strong angular momentum redistribution during the MS; the high efficiency of this mechanism makes the internal rotation profile converge towards an equilibrium profile after only a few percent of the MS time (Zahn 1992; Meynet & Maeder 2000; Maeder & Meynet 2001). While the rotation profiles at the end of the accretion phase essentially reflect the Jaccretion history (see Sect. 3), the MS profiles are expected to be entirely rebuilt by the actions of meridional currents. In fact, the MS equilibrium profile and the corresponding surface velocities of a model of given mass and metallicity depend on the accretion history only through the total amount of angular momentum accreted (Haemmerlé et al. 2013; Granada & Haemmerlé 2014).
In order to show how this angular momentum redistribution impacts our models, we plotted on the lower panel of Fig. 10 the ratio v_{surf}/v_{crit} reached by models with various M_{ZAMS} once they had converged to their MS equilibrium. We see that the stellar surface of all our models spins up between the birthline and the MS equilibrium, with a gain of 0.2–0.3 in v_{surf}/v_{crit}. The equilibrium values of v_{surf}/v_{crit} for the various M_{ZAMS} are all included in the range 40–60%, due to our choice of the Jaccretion history (see Sect. 4.1). For M_{ZAMS}> 20M_{⊙}, since the minimum radius is reached on the birthline, this spinning up is entirely due to angular momentum redistribution by meridional currents. For models at lower masses, the PMS contraction between the birthline and the ZAMS also contributes to this increase by local angular momentum conservation. In order to disentangle these two mechanisms, we added two additional curves on the lower panel of Fig. 10: the blue dashed line indicates the value of v_{surf}/v_{crit} of the same models at the end of the PMS contraction (minimum radius), and the blue dotted line shows the same without the effect of angular momentum transport, computed simply by using v_{surf} × R_{min} = v_{birthline} × R_{birthline}. In other words, the dashed line delimitates the PMS and the MS spinning up, while the dotted line delimitates the effect of local angular momentum conservation and of angular momentum transport. As we see, in the whole mass range, the spinning up is dominated by the angular moment transport from meridional currents. Moreover, in the low and intermediatemass range, meridional currents are efficient enough to achieve convergence towards the MS equilibrium profiles already during the PMS contraction. Thus, during the PMS contraction and the MS evolution, the internal angular momentum transport regulates the rotational history of the star, in contrast to the accretion phase.
Finally, in order to illustrate the convergence process of rotation profiles during the early MS, we computed models starting from the ZAMS with flat rotation profiles, with the same total amount of angular momentum as our models built by accretion. Figure 11 shows the cases where M_{ZAMS} = 9 and 60 M_{⊙}. Despite the differences in the initial surface velocities, we see that models with the same mass and angular momentum converge rapidly towards the same value of v_{surf}/v_{crit}. In the case of models built by accretion, and with highly differential rotation profiles on the ZAMS, meridional currents redistribute the angular momentum from the fast rotating core to the slowly rotating surface, leading to an increase in v_{surf}/v_{crit}. In contrast, for models starting on the ZAMS with solidbody rotation, meridional currents redistribute the angular momentum from the surface to the core. Due to the short timescale of the convergence process, the differences in the rotation profiles do not survive long enough to have a significant impact on further evolution in terms of chemical composition or evolutionary tracks. This result was already described in detail in Haemmerlé et al. (2013). Since it is based on the actions of meridional currents after the accretion phase, the improvements brought to the code since this work have no impact on this conclusion.
Fig. 11 Convergence of the surface velocities towards MS equilibrium. Both panels show the evolution of the ratio v_{surf}/v_{crit} during the early MS as a function of the central massfraction of hydrogen that depicts time along the MS. The upper panel shows the case M_{ZAMS} = 9 M_{⊙} and the lower panel the case M_{ZAMS} = 60 M_{⊙}. On each panel, the blue dashed curve corresponds to the model built by accretion, described in Sect. 4.2, while the grey solid curve indicates a model started on the ZAMS with a flat rotation profile with the same mass and angular momentum as the blue model. The grey dotted horizontal lines indicate the critical limit. 
5. Discussion
5.1. The angular momentum barrier
Stellar models described in Sect. 3 show that smoothJ accretion leads to a limitation in the stellar mass; if the accreted material is dragged by the stellar surface without any braking, the critical rotation limit is reached before the star becomes massive. This angular momentum barrier is independent of the choice of the initial rotation velocity (Sect. 3.2) or of the mass accretion history (Sect. 3.3). Only a change in the Jaccretion history can compensate this effect and overcome any limitation in mass or velocity during the accretion phase. We showed in Sect. 3.4 that the constantj_{accr} assumption with j_{accr} ≃ 1−4 × 10^{18}cm^{2} s^{1} allows for circumvention of the angular momentum barrier. However, the physical conditions that lead to such angular momentum accretion rates remain unknown. How the accreted angular momentum compares with the Keplerian value (20)expected in the accretion disc also remains to be explored.
From the massradius relation of the birthline described in Sect. 4.1 (upper panel of Fig. 10), one can estimate the typical mass and radius of PMS stars accreting at high rates as 10 M_{⊙} and 10 R_{⊙}, respectively. This leads to (21)Comparing this value to the angular momentum effectively accreted (second panel of Fig. 10), we see that j_{accr} remains lower than 10% of the Keplerian angular momentum. The same conclusion holds for the models described in Sect. 3.4. In Appendix B, we show that, indeed, the angular momentum accreted has to be lower than one third of the Keplerian angular momentum. This indicates that the angular momentum barrier can only be circumvented with a strong braking mechanism, efficient enough to remove more than two thirds of the angular momentum from the Keplerian disc.
5.2. The keyrole of the Jaccretion law
Models of Sect. 3 also show that angular momentum transport by shear diffusion and meridional circulation remains weak in the short timescale of the accretion phase, and that the evolution of the rotational properties of accreting stars is dominated by local angular momentum conservation. As a consequence, nearly any rotation profile can be built during the accretion phase by choosing the appropriate Jaccretion history. Indeed, each Lagrangian layer retains essentially the same angular momentum it had when it was accreted, so that the jprofiles reflect the Jaccretion history. Then, the Ωprofiles are given by the jprofiles and the relative contraction of each layer, which is almost independent of rotation and can be taken from nonrotating models. Angular momentum transport by meridional currents can only modify this fact in the very external layers of fast rotators (Sect. 3.4).
An exception to this rule is the case of convective zones, in which angular momentum transport is instantaneous because of the solidbody assumption. Convection appears in two regions in our models, first in the convective envelope before the swelling, then in the convective core after the ZAMS. During the crucial phase of the postswelling KH contraction, all the fast contracting external layers that reach the critical limit in the smoothJ case have been radiative since they were accreted. This explains why a change in the accretion law solves the problem of the angular momentum barrier; if j_{accr} is kept constant, this means that Ω will be small when material is accreted at large radii during the swelling, according to Eq. (8). When the star contracts, the increase of Ω will then not be sufficient for Ω to reach the critical limit.
Interestingly, we notice that for stars that follow the birthline until the ZAMS, all the layers of the convective envelope are eventually incorporated into the convective core (see the isomass in the upper panel of Fig. 10). As a consequence, all the layers of massive stars that are radiative at the end of the accretion phase have been so since they were accreted, and thus they experienced only weak angular momentum transport. So, except for the constraint of solidbody rotation in the convective core, the rotation profiles of massive stars at the beginning of the MS reflect essentially the Jaccretion history.
For low and intermediatemass stars, we showed in Sect. 4.2 that angular momentum transport by meridional currents is strong enough to dominate the rotational history during the PMS contraction that follows the accretion phase. However, the action of these meridional currents simply leads to a convergence of the rotation profiles towards MS equilibrium, and therefore we expect this action to be null if the rotation profile at the end of the accretion phase is close enough to equilibrium.
The freedom in the early MS rotation profile of massive stars has interesting consequences for the evolution of rotation on the MS, in particular for fast rotators and Be stars. Granada & Haemmerlé (2014) presented a grid of MS and postMS models that rotate close to their critical limit during the whole MS. Such models were lacking in previous grids due to the usual assumption of solidbody rotation on the ZAMS. Indeed, as described in Sect. 4.2, with a flat rotation profile on the ZAMS, meridional currents lead to a decrease in the surface velocity during the early MS. Thus even models started on the ZAMS at the critical velocity evolve rapidly towards v_{surf}< 80% v_{crit} (Ekström et al. 2008). In order to produce models that account for the fast rotators observed throughout the MS (Huang et al. 2010), one needs to consider differential rotation upon arrival on the ZAMS. Indeed, the justification of solidbody rotation on the ZAMS is based on the assumption that PMS stars are convective. However, it is well known that large radiative regions develop already during the PMS (Stahler et al. 1980a,b; Hosokawa & Omukai 2009; Hosokawa et al. 2010; see also Paper I), and our computations demonstrate that nonhomologous contraction of the various layers leads to significant differential rotation before the star reaches the ZAMS. The nonflat rotation profiles used by Granada & Haemmerlé (2014) on the ZAMS came from two sources; some were taken from PMS computations (Haemmerlé et al. 2013), performed with the old version of the Geneva code, that were slightly differentially rotating. However, differential rotation in these models was still too low compared to the MS equilibrium profiles, and adhoc profiles were needed to account for the fastest rotators, having v_{surf} ≃ 95% v_{crit} during the whole MS. The results of the present work support the validity of these two types of profiles, and we propose that there exists an angular momentum accretion history that produces such rotation profiles on the ZAMS. We postpone the exact determination of such an angular momentum accretion history to a later study.
5.3. Constraints on PMS evolution from rotation
We showed in Sect. 3.5 that in the constantj_{accr} case, the decrease in v_{surf}/v_{crit} during the accretion phase is more pronounced when using lowentropy RC initial models than highentropy CV models. With the RC initial model, starting at a large fraction of the critical velocity, we reach the highmass range at a low fraction of the critical velocity. A star that reaches 2 M_{⊙} with a RC structure can rarely become a fast rotator once it enters the highmass range, because a ratio v_{surf}/v_{crit}< 1 at 2 M_{⊙} would lead to v_{surf}/v_{crit} ≪ 1 in the highmass range. This effect could be compensated by a change in the angular momentum accretion history (see Sect. 5.2), but we see that the use of the RC initial model reduces the freedom in the Jaccretion history for the formation of massive fast rotators by accretion compared to the CV case.
Moreover, due to their compactness, RC initial models rotate closer to their critical limit compared to CV initial models having the same total amount of angular momentum. In the cases described in Sect. 3.5, we had to assume a slow rotator in the CV case in order to be able to produce a RC initial model having the same angular momentum content and rotating under the critical limit. A RC initial model having the same angular momentum content as the fastest rotators considered in Sect. 3.4, for instance, would exceed the critical limit. In Appendix B, we show that RC models accreting angular momentum according to j_{accr} = 20%j_{K} reach the critical limit at M = 5M_{⊙}. Thus one may wonder if such compact RC models could be formed by accretion without facing the critical limit.
Answering these questions requires following the early accretion phase with a consistent treatment of accretion and rotation. This issue will be the topic of future work, but the present results already provide evidence in favour of our CV initial models.
5.4. Semianalytical interpretation
If one neglects any internal angular momentum transport and the deformation of the star due to rotation, the evolution of the surface velocity is given simply by the accreted angular momentum, according to (22)As in Eq. (8), the factor 2/3 reflects the fact that the material at the surface is distributed over a spherical shell. Using and Eq. (20), one has (23)We note that the fraction 3/2 survives in the righthand side of Eq. (23) because the angular momentum from the disc, which we assume to be confined to the equatorial plan, is redistributed spherically on the stellar surface when it is accreted, according to shellular rotation. Indeed, the fraction 2/3 appears in the expression of j_{surf} (Eq. (22)), but not in the expression of j_{K} (Eq. (20)), therefore it does not cancel in Eq. (23).
Since the stellar mass increases by one or two orders of magnitude between our initial models and massive stars, for constant j_{accr}, the ratio v_{surf}/v_{crit} decreases slightly during the evolution. It remains, however, in the same order of magnitude, thanks to the square root in Eq. (23). This behaviour is similar to that of models described in Haemmerlé et al. (2013), computed with the old version of the code and the smoothJ assumption, where the mean specific angular momentum was also constant. In contrast, however, with the new version of the code, fast rotators in the highmass range can be produced as well by choosing a Jaccretion history in which j_{accr} increases during the evolution, such as the one used in Sect. 4.
If we assume solidbody rotation instead of local conservation of angular momentum, we have (24)Defining the dimensionless parameter (25)that reflects the internal mass distribution, one has (26)If j_{accr} = const., we obtain a similar relation to that in Eq. (23), with a factor 5/2α in front, instead of 3/2. The parameter α is 1 for homogeneous density distribution (∇ρ = 0), and smaller for any realistic structure (∇ρ< 0). Thus, solidbody rotation increases the ratio v_{surf}/v_{crit} compared to the differentially rotating case. Indeed, angular momentum is more centralised in the differentially rotating case than for solidbody rotation, due to the negative Ω gradient, as visible in Fig. 7, and it results in a slower surface rotation.
This fact is visible from the lower panel of Fig. 9. In addition to the evolution of the ratio v_{surf}/v_{crit} for our differentially rotating models (solid lines), we plotted the evolution of v_{surf}/v_{crit} computed with the solidbody assumption, using Ω = J/I (dotted lines). As soon as differential rotation appears, the solidbody case leads to higher surface velocities than in the differentially rotating case. This effect is particularly catastrophic in the RC case, where the solidbody model reaches the critical limit at 5 M_{⊙}. Solidbody rotation could arise in the presence of a strong magnetic field, for instance in the case of an efficient TaylerSpruit dynamo, not considered here. The present analysis shows that, in this case, the critical limit would be reached earlier than in the nonmagnetic case, that is, that the constraint of the angular momentum barrier would be stronger than in our models.
5.5. Comparison with previous studies
Lee & Yoon (2016) studied the evolution of rotation during the accretion phase in the case of Population III stars, considering rates as high as 4 × 10^{3}M_{⊙} yr^{1}. However, differential rotation was not included in their study, and the authors assumed solidbody rotation, postprocessed from computations of accreting stars performed with the MESA code (Paxton et al. 2011, 2013, 2015). The accreted angular momentum was taken as a constant fraction of the Keplerian angular momentum (given by Eq. (20)). Stars accreting at the high rates considered in this work are known to approach the Eddington limit before it has contracted to the ZAMS (Omukai & Palla 2001, 2003). In the presence of rotation, the centrifugal force lowers the upper limit in luminosity, which is compatible with hydrostatic equilibrium. This effect is known as the ΩΓlimit (Maeder & Meynet 2000). The models of Lee & Yoon (2016) reached the ΩΓlimit during the swelling, which occurs at masses between 20 and 40 M_{⊙} at this accretion rate, preventing further accretion and limiting the mass of stars that can form by accretion.
Our models at solar metallicity show that differential rotation cannot be neglected during the swelling phase. The semianalytic considerations of Sect. 5.4 show that differential rotation can significantly reduce the ratio v_{surf}/v_{crit}. We showed that solidbody rotating models reach the critical limit if the swelling exceeds 100 R_{⊙}, but that differential rotation avoids such a catastrophic end. It is thus necessary to take into account differential rotation in order to test the validity of such mass limitations.
6. Conclusions
After having improved the treatment of accretion in the Geneva code (Sect. 2.1 and Appendix A; see also Paper I), we described in the present work the PMS evolution of solar metallicity stars with accretion and rotation by considering various accretion laws for the mass and the angular momentum (Sect. 3). Our main results can be summarised as follows:

1.
Angular momentum transport by shear and meridionalcurrents inside the radiative layers of the star remains weak duringthe short accretion timescale (Sect. 3.1). Onlyconvective transport is efficient (solidbody assumption), and theevolution of the rotational properties in radiative regions isdominated by local angular momentum conservation. Sincelarge radiative regions develop during the accretion phase, theinternal rotation profiles during this phase essentially reflect theangular momentum accretion history. The highlynonhomologous PMS contraction leads, in general, tosignificant differential rotation in the stellar interior.

2.
Under the assumption of smooth angular momentum accretion, the new version of the code leads to a limitation in mass instead of a limitation in rotation velocity (Sect. 3.1). This implies that if the accreted material is dragged by the stellar surface without braking, the forming star reaches the critical limit before it can significantly enter into the highmass range. This is due to the rapid contraction of the stellar surface after the PMS swelling. When the critical rotation limit is reached, accretion stops, thus preventing the formation of massive stars. This angular momentum barrier is independent of the choice of the initial rotation velocity (Sect. 3.2) or of the mass accretion history (Sect. 3.3).

3.
Only a change in the angular momentum accretion history can circumvent the angular momentum barrier, and overcome any limitation in mass or velocity during the accretion phase. A careful choice of the Jaccretion history allows for production of stars of any mass and velocity compatible with the structure equations. Using the constantj_{accr} assumption, the ratio v_{surf}/v_{crit} remains of the same order of magnitude during the accretion phase, similarly as with the old version of the code and smoothJ accretion (Sect. 3.4). Angular momentum accretion histories compatible with massive star formation by accretion imply an orbital velocity in the inner disc that is lower than one third of the Keplerian value (Sect. 5.1 and Appendix B). We conclude thatmassive star formation by accretion requires an efficient braking mechanism in the inner accretion disc in order to circumvent the angular momentum barrier.

4.
For angular momentum accretion histories that allow massive stars to form, the internal rotation profiles during the accretion phase decrease outwards (Sects. 3.4 and 4.1). The degree of differential rotation reaches its maximum after the swelling, with a core rotating approximately seven times faster than the surface. Then, differential rotation is reduced as the stellar surface contracts, but survives until the end of our computations, with a core that rotates two to three times faster than the surface as the star reaches a MS structure. Such differential rotation allows the star to reach higher masses than in the case of solidbody rotation that would eventually arise in the presence of a strong magnetic field (Sect. 5.4).

5.
The compact initial conditions, with a low entropy content, that lead to a significant swelling during the accretion phase, reduce the freedom in the angular momentum accretion histories that allow massive fast rotators to form (Sects. 3.5 and 5.3). This result supports the validity of our extended initial models with high entropy content, that avoid a significant PMS swelling (see Paper I).

6.
The accretion history during the PMS phase has no significant impact on the MS and postMS evolution (Sect. 4.2). Models based on various PMS scenarios converge to an internal rotation structure that depends only on their mass, their chemical composition, and their total amount of angular momentum, after only a few percent of the MS timescale.

7.
Thanks to the low efficiency of angular momentum transport by shear and meridional currents, very different rotation profiles on the ZAMS are possible, strongly depending on the angular momentum accretion history the star experienced (Sect. 5.2). This fact supports the validity of previously published models that rotate close to their critical limit during their whole MS phase.
As in Paper I: Z = 0.014, with the abundances of Asplund et al. (2005) and Cunha et al. (2006), and a deuterium mass fraction of 5 × 10^{5} (Bernasconi & Maeder 1996; Norberg & Maeder 2000; Behrend & Maeder 2001; Haemmerlé et al. 2013).
Acknowledgments
Part of this work was supported by the Swiss National Science Foundation. L.H. and R.S.K. were supported by the European Research Council under the European Community’s Seventh Framework Programme (FP7/2007 – 2013) via the ERC Advanced Grant “STARLIGHT: Formation of the First Stars” (project number 339177).
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Appendix A: Effects of the improvements in the code
Here we describe the effects of the improvements in the code that are related to rotation. We consider the same physical conditions as in Sect. 3.1: the initial model is given by Eqs. (10) and (11), mass is accreted at 10^{5}M_{⊙} yr^{1} (Eq. (9)) and angular momentum according to the smoothJ assumption, as in Haemmerlé et al. (2013). The model computed with these inputs and the new version of the code has been described in Sect. 3.1. Here we compare this model with the equivalent one computed with the old version of the code, using the same physical inputs.
Fig. A.1 Global rotational properties of the models described in Appendix A. Upper panel: angular momentum accretion rate and lower panel: ratio v_{surf}/v_{crit}, with the critical limit indicated by the dotted horizontal grey line. 
The global rotational properties of these two models are compared in Fig. A.1. Both models start their evolution at v_{surf} = 0.42 km s^{1} = 0.28% v_{crit}, according to Eq. (11). In the model computed with the old version of the code, with the artificial loss of angular momentum, the surface velocity remains in the same order of magnitude during the whole PMS, with values in the range 0.25 km s^{1}<v_{surf} ≲ 1.05 km s^{1}. The corresponding angular momentum accretion rate is constant during the evolution (dJ/ dM ≃ 3 × 10^{15}cm^{2} s^{1}). This result is in agreement with the case described in Haemmerlé et al. (2013), corresponding to a different mass accretion rate and a higher initial velocity (Ω_{ini} = 2.1 × 10^{5} s^{1}, that is v_{surf}/v_{crit} = 80%).
However, the behaviour of the model computed with the new version of the code, without any artificial loss of angular momentum, is drastically different. As described in Sect. 3.1, the surface velocity does not remain in the same order of magnitude, but increases by several orders of magnitude, in particular during the postswelling contraction. The corresponding angular momentum accretion rate is no longer constant, but increases with mass and time, by two orders of magnitude between 0.7 and 6 M_{⊙}. This illustrates the fact that in cases of smoothJ accretion, the angular momentum accretion rate depends itself on the evolution of rotation in the model.
Fig. A.2 Rotation profiles of the models described in Appendix A, at M = 2, 4 and 6 M_{⊙}. Upper panel: jprofiles and lower panel: Ωprofiles. 
Figure A.2 shows the internal rotation profiles of these two models: The jprofiles in the upper panel and the Ωprofiles in the lower panel. With the old version of the code, the specific angular momentum decreases with time in each layer, that is, for each fixed value of the Lagrangian coordinate. This is the effect of the artificial loss of angular momentum described in Sect. 2. With the new version of the code, the angular momentum is locally conserved in each radiative layer, which leads to Ωprofiles that increase outwards, as described in Sect. 3.1. In the old model, the artificial loss of angular momentum is more important in the external regions than in the core (see Haemmerlé 2014). As a consequence, the Ωprofiles decrease outwards in this case. As described in Haemmerlé et al. (2013), this leads to a rotation profile on the ZAMS that is close to the equilibrium profile with respect to meridional circulation during the MS evolution.
Appendix B: Accretion of angular momentum at a constant fraction of the Keplerian value
The models described in Sect. 3.4, that circumvent the angular momentum barrier, correspond to an angular momentum accreted that is lower than 10% of the Keplerian angular momentum j_{K} (Sect. 5.1). Here we estimate the upper fraction of j_{K}the star can accrete without facing the angular momentum barrier. We aim to compute models accreting angular momentum at a constant fraction of j_{K}. However, as in Sect. 3.4, we cannot freely control the accretion of J in this case; in particular when large external regions of the star are convective. Figure B.1 shows the stellar structure, the angular momentum accretion rate, and the ratio v_{surf}/v_{crit} for two models accreting mass at a rate of 10^{3}M_{⊙} yr^{1}. The first one is computed from the CV initial structure, and the second one from a RC structure (see Sect. 3.5).
Fig. B.1 Internal structure (upper panel), angular momentum accretion rate (middle panel), and ratio v_{surf}/v_{crit} (lower panel) of the models described in Appendix B. Lefthand column shows the properties of the models started from a CV initial structure, while the righthand column corresponds to the RC initial structure. On the top panel, the upper solid curve is the stellar radius, while convective and radiative zones are shown in dark and light grey, respectively. The dotted black curves are isomass at intervals of 1 M_{⊙}. In the middle panel, the coloured lines indicate the angular momentum effectively accreted by the models, and the black dotted curves show the value of j_{accr} corresponding to the indicated fraction of j_{K}. On the lower panel, the horizontal dotted line indicates the critical limit. 
The angular momentum accreted in the CV model is always lower than 35% of j_{K}. Without any angular momentum transport, the surface velocity would thus remain approximately one third of v_{crit}. However, during the early phase, the star is fully convective and angular momentum is instantaneously redistributed in the stellar interior. The assumption of solidbody rotation leads to outwards transport of angular momentum that produces an increase in v_{surf}. As evolution proceeds, the ratio v_{surf}/v_{crit} increases monotonously and reaches the critical limit at a mass of 3.4 M_{⊙}, before the formation of the radiative core. This example shows that the material of the accretion flow has to be slowed down to under one third of the Keplerian velocity expected in the disc. We emphasise that this value is only an upper limit. The exact determination of the fraction of angular momentum that must be removed from the Keplerian disc will be the topic of a forthcoming paper. We note, however, that according to Eq. (21), the fastest rotator of Sect. 3.4 accretes angular momentum at ~ 10%j_{K} without reaching the critical limit.
Since this limitation is due to the instantaneous redistribution of J while the star is fully convective, one wonders whether the RC models allow for circumvention of this limitation. The righthand side of Fig. B.1 shows that this is not the case. Even with j_{accr}< 20% j_{K}, the angular momentum transport in the small external convective zone leads the star to the critical limit soon after 5 M_{⊙}.
All Figures
Fig. 1 Evolution of the internal structure, the angular momentum accretion rate, and the equatorial surface velocity of the testmodel at low massaccretion rate described in Sect. 3.1, as a function of the increasing stellar mass, which is a timecoordinate in the case of accretion. Upper panel: radius (blue curve) and the internal structure, with convective zones in dark grey and radiative zones in light grey. The dark grey dotted curves are isomass of M_{r} = 1, 2, 3,..., M_{⊙}. Second panel: angular momentum accretion rate in logarithm of . Third panel: surface velocity (at the equator) and the fourth panel shows the ratio of the surface velocity to the critical velocity. (The critical limit is indicated by the horizontal grey dotted line.) 

In the text 
Fig. 2 Internal rotation profiles of the model at low massaccretion rate described in Sect. 3.1 for evolutionary stages M = 2, 4, and 6 M_{⊙}, as a function of the Lagrangian coordinate M_{r}. The upper panel shows the profiles of the specific angular momentum while the lower panel shows the angular velocity Ω. 

In the text 
Fig. 4 As in Fig. 1 (without v_{surf}), for the model with Ṁ = 10^{3}M_{⊙} yr^{1} and Ω_{ini} = 10^{8} s^{1}, described in Sect. 3.3. The isomass corresponds to M_{r} = 2, 4, 6,..., M_{⊙}. 

In the text 
Fig. 5 As in Fig. 1 (without v_{surf}), for the model with CH accretion and Ω_{ini} = 10^{8} s^{1}, described in Sect. 3.3. 

In the text 
Fig. 6 Varying the angular momentum accretion history, for Ṁ = 10^{3}M_{⊙} yr^{1}. Upper panel: internal structure of the nonrotating model: the upper curve is the stellar radius, the dark grey regions are convective, the light grey is radiative, and the dotted lines are iosmass of 2, 4, 6, 8,..., M_{⊙}. Second panel: three Jaccretion histories considered and the third one, specifically, shows the evolution of v_{surf}/v_{crit} for the corresponding models (the grey dotted horizontal line indicates the critical limit), and bottom panel: deformation of the star due to rotation (R_{eq} and R_{pol} are the equatorial and polar radii, respectively). 

In the text 
Fig. 7 Internal rotation profiles of the model with Ṁ = 10^{3}M_{⊙} yr^{1} and j_{accr}≃ 4 × 10^{18}cm^{2} s^{1} (fastest rotator of Fig. 6) for M = 5, 10, 15, 20, 25, 30 M_{⊙}, as a function of the Lagrangian coordinate M_{r}. Upper panel: profiles of the specific angular moment , and second panel: profiles of the angular velocity Ω. On the bottom panel timescales for angular momentum transport by shear diffusion and meridional circulation at M = 15M_{⊙}, and compare it with the PMS timescale M_{ZAMS}/Ṁ≃ 35 000 yr. The arrows indicate the direction of the angular momentum transport by meridional currents, outwards or inwards. 

In the text 
Fig. 8 Internal structure of the initial models described in Sect. 3.5. Upper panel: entropy profile and lower panel: Ωprofile. Entropy is computed from an arbitrary reference value s_{0} that corresponds to the high entropy CV model. In each panel, the boundary between convection and radiation in the lowentropy RC model is indicated by a dot. 

In the text 
Fig. 9 Evolution of the models described in Sect. 3.5, with Ṁ = 10^{3}M_{⊙} yr^{1} and j_{accr} ≃ 10^{18} cm^{2} s^{1}, started from the CV and the RC models (black and green lines, respectively). Upper panel: stellar radius, second panel: moment of inertia, third panel: accretion of angular momentum, and the lowest panel the ratio of the surface rotation velocity to the critical velocity. In the upper panel, the solid lines correspond to the stellar radius and the dotted lines indicate the location of the layer that encloses 90% of the actual stellar mass. In the third panel, the grey dotted line is the ideal value of j_{accr} = 10^{18} cm^{2} s^{1} while in the lowest panel, the grey dotted line indicate the critical limit and the coloured dotted lines indicate the evolution of v_{surf}/v_{crit} with the assumption of solidbody rotation (see Sect. 5.4). 

In the text 
Fig. 10 Properties of the birthline described in Sect. 4.1. Upper panel: stellar radius (upper blue curve) and the internal structure, with convective regions in dark grey, radiative regions in light grey, and isomass as dotted curves. Second panel: accretion of specific angular momentum (in logarithm of cm^{2} s^{1}): the black dotted line is the value given by Eq. (19) and the solid blue line indicates the angular momentum effectively accreted. Third panel: angular velocity at the surface and in the centre. The lower panel shows the ratio v_{surf}/v_{crit} (lower thick solid blue line). The filled squares connected by the thin blue line indicate the values of v_{surf}/v_{crit} reached by the models at constant mass computed from the birthline once they have converged to their MS equilibrium (see Sect. 4.2). The blue dashed line shows the values of v_{surf}/v_{crit} of the same models when they reach their minimum radius corresponding to the ZAMS. We also added the value of v_{surf}/v_{crit} these models would have at the minimum radius if angular momentum was locally conserved (blue dotted line). The grey dotted horizontal line indicates the critical limit. 

In the text 
Fig. 11 Convergence of the surface velocities towards MS equilibrium. Both panels show the evolution of the ratio v_{surf}/v_{crit} during the early MS as a function of the central massfraction of hydrogen that depicts time along the MS. The upper panel shows the case M_{ZAMS} = 9 M_{⊙} and the lower panel the case M_{ZAMS} = 60 M_{⊙}. On each panel, the blue dashed curve corresponds to the model built by accretion, described in Sect. 4.2, while the grey solid curve indicates a model started on the ZAMS with a flat rotation profile with the same mass and angular momentum as the blue model. The grey dotted horizontal lines indicate the critical limit. 

In the text 
Fig. A.1 Global rotational properties of the models described in Appendix A. Upper panel: angular momentum accretion rate and lower panel: ratio v_{surf}/v_{crit}, with the critical limit indicated by the dotted horizontal grey line. 

In the text 
Fig. A.2 Rotation profiles of the models described in Appendix A, at M = 2, 4 and 6 M_{⊙}. Upper panel: jprofiles and lower panel: Ωprofiles. 

In the text 
Fig. B.1 Internal structure (upper panel), angular momentum accretion rate (middle panel), and ratio v_{surf}/v_{crit} (lower panel) of the models described in Appendix B. Lefthand column shows the properties of the models started from a CV initial structure, while the righthand column corresponds to the RC initial structure. On the top panel, the upper solid curve is the stellar radius, while convective and radiative zones are shown in dark and light grey, respectively. The dotted black curves are isomass at intervals of 1 M_{⊙}. In the middle panel, the coloured lines indicate the angular momentum effectively accreted by the models, and the black dotted curves show the value of j_{accr} corresponding to the indicated fraction of j_{K}. On the lower panel, the horizontal dotted line indicates the critical limit. 

In the text 
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