Migration and gas accretion scenarios for the Kepler 16, 34 and 35 circumbinary planets
Key Words.:
accretion, accretion disks – planetary systems: formation – hydrodynamics – methods: numericalAbstract
Context:Several circumbinary planets have been detected by the Kepler mission. Recent work has emphasized the difficulty of forming these planets at their observed locations due to perturbations by the binary. It has been suggested that these planets formed further out in their discs in more quiescent environments and migrated in to locations where they are observed.
Aims:We examine the orbital evolution of planets embedded in circumbinary disc models for the three systems Kepler16, Kepler34 and Kepler35. The aims are: to explore the plausibility of a formation scenario in which cores form at large distances from the binaries and undergo inward migration and gas accretion as the gas disc disperses; to determine which sets of disc parameters lead to planets whose final orbits provide reasonable fits to the observed systems.
Methods:Using a grid–based hydrodynamics code we performed simulations of a close binary system interacting with circumbinary discs with differing aspect ratios, , and viscous stress parameters . Once the binary+disc system reaches quasiequilibrium we embed a planet in the disc and examine its evolution under the action of binary and disc forces. We consider fullyformed planets with masses equal to those inferred from Kepler data, and lowmass cores that migrate and accrete gas while the gas disc is being dispersed.
Results:A typical outcome for all systems is stalling of inward migration as the planet enters the tidallytruncated inner cavity formed by the binary system. The circumbinary disc becomes eccentric through interaction with the binary, and the disc eccentricity forces the planet into a noncircular orbit. For each of the Kepler16b, Kepler34b and Kepler35b systems we obtain planets whose parameters agree reasonably well with the observational data, but none of our simulations are able to produce highly accurate fits for all orbital parameters.
Conclusions:The final orbital configuration of a circumbinary planet is determined by a delicate interplay between the detailed stucture of the circumbinary disc and the orbital parameters of the planet as it migrates into the inner disc cavity. Simplified simulations such as those presented here provide support for a formation scenario in which a core forms, migrates inward and accretes gas, but accurate fitting of the observed Kepler systems is likely to require disc models that are significantly more sophisticated in terms of their input physics.
1 Introduction
Among the thousands of planet candidates discovered by Kepler, at the time of writing 6 of them are circumbinary planets which orbit around both components of a close binary system on a socalled Ptype orbit. Kepler16b was the first circumbinary planet discovered with Kepler (Doyle et al. 2011). It is a Saturnmass planet with nearcircular orbit and semimajor axis AU (measured from the centre of mass of the binary). The binary harbouring Kepler16b has semimajor axis AU, eccentricity and mass ratio , where and are the masses of the primary and secondary stars respectively. Interestingly, Kepler16b is found to orbit just outside the longterm stability limit located at AU from the binary (Holman & Wiegert 1999). Two additional transiting circumbinary planets have been reported by Welsh et al. (2012) around Kepler34 and Kepler35: binary systems with stellar binary periods of and days, respectively. Kepler34b has orbital period days and mass ratio , where and is the planet mass. Kepler35b has orbital period days and mass ratio . The binary and planet parameters for these three systems are summarized in Table 1. More recent detections include the Neptunesized circumbinary planet Kepler38b (Orosz et al. 2012a), a system of 2 planets around Kepler47 (Orosz et al. 2012b), and a transiting circumbinary planet around KIC 4862625 (Schwamb et al. 2013).
These circumbinary planets are all found to have highly aligned orbit planes with respect to the central binaries. Although transit photometry is a detection technique biased toward finding coplanar orbits (Winn et al. 2011), this nonetheless suggests that these planets formed within a coplanar circumbinary disc. For Kepler16b, this is further supported by the fact that the spin of the primary is aligned with the angular momentum of the binary+planet system (Winn et al. 2011). Moreover, this is also consistent with detections of circumbinary discs around spectroscopic binaries like DQ Tau, AK Sco and GW Ori. In GG Tau, the circumbinary disc has been directly imaged and has revealed the presence of an inner cavity due to the tidal torques exerted by the central binary (Dutrey et al. 1994).
Early studies of the dynamics of planetesimals embedded in circumbinary discs adopted simple axisymmetric disc models, and showed that eccentric orbits induced by the tidal influence of the binary companions would experience pericentre aligment due to gas drag forces (Scholl et al. 2007). In principle this can reduce the collision velocities between planetesimals, but pericentre alignment is sizedependent leading to the expectation that collisions within a swarm consisting of a range of planetesimal sizes may be erosive (Scholl et al. 2007). Moreover, nonaxisymmetric structures in the disc such as spiral density waves or global eccentric modes may also lead to large impact velocities, especially if the gravitational field of the disc is included in the evolution of planetesimal orbits (Marzari et al. 2008; Kley & Nelson 2010).
Regarding the circumbinary planets discovered with Kepler, Paardekooper et al. (2012) recently performed Nbody simulations of planetesimal accretion in these systems, including planetesimal formation and dust accretion. They showed that the large eccentricities reached by the planetesimals make it difficult to form these planets insitu. A similar conclusion was drawn by Meschiari (2012) who found that for Kepler16b, planetesimal accretion might be inhibited interior to AU. Both studies indicate that these planets formed further out in the disc, in a more accretionfriendly environment, and migrated inward to their present location through Type I (Ward et al 1997, Tanaka et al. 2002) and/or Type II migration (e.g. Lin & Papaloizou 1986; Nelson et al. 2000).
The evolution of Earthmass bodies embedded in a circumbinary disc and undergoing Type I migration was examined by Pierens & Nelson (2007). They found that the inward drift of a protoplanet can be stopped near the edge of the cavity formed by the binary due to the strong positive corotation torque there counterbalancing the Lindblad torque (Masset et al. 2006). The orbital evolution of Jovian mass planets embedded in circumbinary discs was studied by Nelson (2003) and subsequently by Pierens & Nelson (2008). These authors found that the typical evolution of Saturnmass planets involves inward migration until the planet eccentricity becomes high enough to induce a torque reversal and the subsequent outward migration of the planet. This effect makes Saturnmass planets evolve on a stable orbit, at a safe distance from the central binary. Giant planets with masses of , however, generally undergo close encounters with the binary and are subsequently completely ejected from the system. We notice that the values for the inferred masses of the circumbinary planets discovered with Kepler are surprisingly consistent with these results.
In this paper, we present hydrodynamic simulations of the orbital evolution of planets embedded in circumbinary disc models designed to mimic the protoplanetary discs that existed in the Kepler16, Kepler34 and Kepler35 systems during the epoch of planet formation. The models we adopt are by their nature very simple: flat 2D locally isothermal discs with constant values in which the accretion stress is modelled using the standard alpha prescription (Shakura & Sunyaev 1973). The aim of this work is to examine the general plausibility of the ideas presented in our previous papers that the orbital configuration of circumbinary planets is determined through their interaction with the circumbinary disc, which develops an inner cavity and becomes eccentric through tidal interaction with the central binary. In principle, with sophisticated disc modelling that includes processes such as magnetohydrodynamic turbulence, time dependent radiative heating of the disc by the stellar components, selfgravity, heat transport and a realistic equation of state, one could attempt to fit the Kepler observations of circumbinary planets and thereby constrain the nature of the circumbinary discs in which the planets formed and migrated. Such a project is beyond current capabilities so we adopt the less ambitious aim of obtaining decent agreement between our simplified simulations and the observed Kepler circumbinary planets to support the plausibility of the general core formation, migration and gas accretion model for these planets.
We consider two basic scenarios: (i) formation of the planet at large distance from the central
binary followed by migration to a final orbit close to the central binary without further mass growth; (ii) formation of a 20 M core
at large distance that migrates inward through type I migration and then accretes gas once migration is halted, and before disc dispersal determines its
final mass and orbit. We examine the outcome of simulations as a function of the adopted disc parameters
(; viscous parameter; discdispersal time scale).
We find that different disc models are needed to produce decent approximations to the observed parameters of each of the
Kepler16, Kepler34 and Kepler35 systems. For example, a circumbinary disc with and reproduces
Kepler34b reasonably well, whereas and provide decent agreement with the Kepler35b data.
For Kepler16b, a close fit to the observed parameters is obtained using a disc model with and ,
although all our simulations have difficulty in reproducing the very low eccentricity reported for this system.
For each system we find that the planet migrates into the tidally truncated disc cavity created by the
binary before halting, as anticipated by Nelson (2003) and Pierens & Nelson (2007; 2008). In the case of Kepler16b,
halting of migration occurs when the amount of local gas in the cavity becomes too small to make the planet migrate
further in; whereas for Kepler34b, Kepler35b, this arises once the planet eccentricity becomes high enough to
induce a torque reversal.
This paper is organized as follows. In Sect. 2, we present the hydrodynamic model. In Sect. 3, we discuss results concerning binarydisc interactions. Results of simulations with fullyformed planets are presented in Sect. 4, and in Sect. 5 we examine the scenario in which a lowmass embryo grows by accreting gas from the disc once it has undergone substantial migration. Finally we discuss our results and draw our conclusions in Sect. 6.
2 The hydrodynamical model
2.1 Numerical method
We adopt a 2D disc model in which all physical quantities are vertically averaged and work in polar coordinates with the origin located at the centre of mass of the binary. The equations governing disc evolution and the binary plus planet system can be found in Pierens & Nelson (2007). The simulations presented here were performed using the GENESIS numerical code which solves the equations for the disc using an advection scheme based on the monotonic transport algorithm (Van Leer 1977). This code has been employed in numerous previous studies of planet formation in circumbinary discs (Pierens & Nelson 2007; 2008a; 2008b).
Evolution of the planet and binary orbits is computed using a fifthorder RungeKutta integrator (Press et al. 1992). For moderate values of disc viscosity, exchange of angular momentum with the disc can lead to significant modification of the binary orbital elements, and it is generally expected that shrinking of the binary separation plus growth of the binary eccentricity will result from the resonant interaction between the disc and binary (Pierens & Nelson 2007). Here, since we want to reproduce as close as possible the observed properties of the Kepler circumbinary planets, the force exerted by the disc onto the binary is not included in the evolution equations, so that the binary orbital elements remain fixed in the course of the simulations with values corresponding to the observed ones.
We adopt computational units such that the total mass of the binary , the gravitational constant and the radius in the computational domain corresponds to AU. When presenting simulation results we report time in units of the binary orbital period .
The simulations employ radial grid cells uniformly distributed between , where is the binary semimajor axis, and (5 AU), and azimuthal grid cells.
2.2 Initial conditions
The initial disc surface density profile is chosen to be where was defined such that the disc contains of the total mass of the binary within AU and is a gap function which is employed to model the inner cavity that is expected to be formed as a result of binarydisc interactions. Following Gunther et al. (2004), we set:
where is the estimated gap size (Artymowicz & Lubow 1994). We adopt a locally isothermal equation of state (this assumption is discussed and justified in Sect. 5.3) with temperature profile given by where and is the temperature at . This corresponds to a disc with constant aspect ratio for which we consider values of , 0.05 and 0.07. For a fiducial run with , the Toomre parameter , where is the epicyclic frequency and the sound speed, is estimated to be at the disc inner edge and at the disc outer edge, which implies that we can safely ignore selfgravity in this work. Neglecting effects resulting from selfgravity is further justified by the recent results of Marzari et al. (2013) who found that for similar values of the Toomre parameter, including selfgravity does not significantly affect the shape of the circumbinary disc for binary parameters corresponding to Kepler16.
The anomalous viscosity in the disc, which probably arises from MHD turbulence, is modelled using the standard alpha prescription for the effective kinematic viscosity (Shakura & Sunyaev 1973) where is the disc scale height. In this work, we use values of , and .
The binary semimajor axis , eccentricity and mass ratio , which remain fixed in the course of the simulations, are set to match the binary orbital elements obtained from Kepler observations. Data for Kepler16 have been taken from Doyle et al. (2011) and parameters for Kepler34 and Kepler35 have been taken from Welsh et al. (2012). We remind the reader that for the three systems, the binary and planet parameters inferred from Kepler data can be found in table .
Planet evolution is initiated on a circular orbit with semimajor axis chosen to be outside the disc inner cavity and in a region where the local disc eccentricity is . For each disc model, we performed one simulation in which the planet mass ratio is equal to the observed value and remains constant, and a second run in which a 20 M embryo is allowed to accrete gas from the disc. In the latter the onset of gas accretion occurs once migration of the lowmass embryo allows it to reach an orbit where migration halts because the net time averaged disc torque equals zero. Following Kley (1999), accretion by the protoplanet is modelled by removing a fraction of the gas located inside the Hill sphere during each time step, and this mass is added to the planet (e.g. Nelson et al. 2000; Pierens & Nelson 2008). The gas removal rate is chosen such that the accretion timescale onto the planet is , where is the orbital period of the planet and is a free parameter.
When calculating the torque exerted by the disc on the planet, we exclude the material contained within a distance from the planet using a Heaviside filter, where is the Hill radius. Such a value is consistent with the one that is recommended by Crida et al. (2009) to obtain an accurate estimation of the migration rate. Moreover, we set the softening parameter for the gravitational potential to .
Kepler 16  Kepler 34  Kepler 35  

()  
()  
()  
(AU)  
(AU)  
2.3 Boundary conditions
At the inner edge of the computational domain we use a closed, reflecting boundary condition. Because the inner boundary is located deep inside the tidally truncated cavity, there is no evidence of wave reflection at the boundary. In order to test the dependence of our results against the choice of boundary condition, we have also employed in some runs a viscous outflow boundary condition (Pierens & Nelson 2008), where the radial velocity in the ghost zones is set to , where is the gas drift velocity due to viscous evolution (assuming steady mass flow) and is a free parameter which was set . At the outer radial boundary, we employ a wavekilling zone for (4.2 AU) to avoid wave reflection/excitation at the disc outer edge (de ValBorro et al. 2006). The impact of this wavekilling zone on the disc shape and eccentricity is expected to be small since, as we will see shortly, the disc is almost circular well inside the wavekilling zone (see Fig. 3 below).
3 Evolution of the binarydisc system
3.1 Evolution of the disc eccentricity
Before presenting simulations of the evolution of embedded circumbinary planets, we first examine briefly the evolution of the binarydisc system and the growth of disc eccentricity. This is not intended to be an exhaustive analysis of this issue as our primary concern in this paper is the evolution of circumbinary planets. We will present a more detailed analysis of the evolution of circumbinary discs in a future publication, where we will consider the influence of radiative processes, selfgravity, binary mass ratios and binary eccentricities.
The left panel of Fig. 1 shows the time evolution of the disc eccentricity for the three systems, where is defined as (Pierens & Nelson 2007):
(1) 
In the previous equation, is the eccentricity of a fluid element computed at the center of each grid cell and the surface area of one grid cell. For each run, the disc eccentricity initially increases and then reaches a saturated value once viscous damping equilibrates the eccentricity forcing rate due to the binary. The observed oscillations in the disc eccentricity arise because the binary longitude of pericentre maintains a constant value while the disc librates with a libration amplitude of degrees. This is illustrated in Fig. 2 which shows the time evolution of the disc longitude of pericentre for the Kepler16 run with and , where is defined by:
(2) 
is the longitude of pericentre of a fluid element evaluated at the center of each grid cell. The fact that the eccentricity oscillation amplitudes are higher in models with is likely due to pressure effects which tend to reduce the prograde precession rate of the disc.
We observe a clear tendency for the final value of to increase with increasing . The Kepler34 run with is the one anomaly, which can perhaps be explained by the smaller viscous stress leading to weaker damping of the locally generated eccentricity at large radius. We leave further investigation of this issue for the future publication mentioned at the beginning of this section.
Comparing the upper and lower panels of Fig. 1 for Kepler16 and Kepler35, where the binaries
have similar eccentricities but different mass ratios, reveals that the saturated value of the disc eccentricity is
almost independent of the binary mass ratio. For example, for our fiducial disc model with and ,
the steady state value for the disc eccentricity is in the Kepler16 run while for Kepler35.
Comparing the middle and lower panels for Kepler34 and Kepler35, however, where the binaries have
similar values for but very different eccentricities, demonstrates that the final value for strongly depends
on the binary eccentricity. Not surprisingly, it is found to be higher in Kepler34 runs with, for example, a stationary value of
reached in the fiducial run with and . Given that the value for the disc eccentricity is
closely related to the size of the inner cavity, as we will see shortly, this is in good agreement with the results of
Artymowicz & Lubow (1994) which suggest that the gap size is strongly dependent on the binary eccentricity but depends weakly
on the binary mass ratio.
An issue that needs to be investigated is how the final value for the disc eccentricity compares with the expected forced eccentricity resulting from the secular interaction with the binary. The forced eccentricity at radius is given by (Moriwaki & Nakagawa 2004):
(3) 
For the Kepler16 system, this gives at AU while for Kepler34 and Kepler35 which have mass ratios close to unity, the forced eccentricity is much lower ( at AU). Except for the Kepler16 run with and , it therefore appears that the saturated value for is generally much higher than the forced eccentricity, which is in good agreement with the results of Pelupessy & Portegies Zwart (2013). This indicates that the contribution to the disc eccentricity growth from secular interaction is minimal.
The right panel of Fig. 1 displays the steadystate disc surface density profile for all calculations, timeaveraged over binary orbits. As the values for and are decreased the inner cavity deepens and the cavity edge steepens. Not surprisingly there also appears a general trend for the location of the density peak to scale with the disc eccentricity. Here, we find that can be reasonably well approximated by the following fitting relation:
(4) 
3.2 Origin of the disc eccentricity
Previous studies of circumbinary discs (e.g. Papaloizou et al. 2001; Pierens & Nelson 2007) have shown that interaction with the binary can cause the disc to become eccentric. As we have discussed above, the forced eccentricity of the disc due to secular interaction with the binary should be small. For a circular binary, Papaloizou et al. (2001) have shown that the origin of the disc eccentricity involves a parametric instability that causes a spiral wave to be launched at the eccentric Lindblad resonance. This instability is generated by nonlinear mode coupling between an initial eccentric disturbance in the disc and the component of the binary potential. This produces a wave with pattern speed that is launched at the Lindblad resonance. The wave transports angular momentum outward, causing the growth of disc eccentricity (Papaloizou et al. 2001). The mechanism at play is very similar to that described by Lubow (1991) in application to superhump phenomena in close binary systems where the disc orbits one component of the binary system. In this case a small binary mass ratio () allows the Lindblad resonance to be present in the disc, leading to the growth of disc eccentricity through a similar instability.
To explore the origin of the disc eccentricity observed in Figs. 1 and 3 we have conducted a number of test calculations. The aim of this study is simply to explore the primary influences on the growth of the eccentricity. In a future paper we will provide an indepth analysis of disc eccentricity growth in circumbinary systems. The findings of our modest present study may be summarised as follows:

Simulations of circumbinary discs with binary mass ratios equal to those in the Kepler16 and 35 systems typically show the growth of substantial disc eccentricity when the binary eccentricity is set to zero. This clearly demonstrates that nonlinear mode coupling and the 3:1 Lindblad resonance play an important role.

Simulations were performed for circular binary systems where the inner boundary of the computational domain was placed outside the location of the 3:1 resonance. Disc eccentricity growth was not observed in these cases, confirming the conclusion in the previous paragraph.

Simulations were performed for binary systems similar to Kepler34 with the inner boundary of the computational domain placed between the locations of the 3:1 and 4:1 Lindblad resonance. Strong disc eccentricity growth was observed in this case, suggesting that nonlinear mode coupling involving higherorder terms in the potential of the binary also cause the growth of disc eccentricity, at least for the highly eccentric Kepler34 binary system.
When both the disc eccentricity and surface density profile have reached a quasi steadystate, we include a planet
that interacts gravitationally with both the binary and the circumbinary disc. This planet initially evolves on a
circular orbit at AU in Kepler16 and Kepler35 runs while the initial semimajor axis
AU in Kepler34 runs. For the three systems, we tested two different scenarios:
(i) We first considered the case of a fullyformed planet for which the planet mass is set to the observed value.
For Kepler16b, this corresponds to a mass ratio , and for Kepler34b and Kepler35b and
, respectively (see Table ).
(ii) We then performed a series of simulations in which the planet mass ratio is . In that case,
the interaction with the disc is linear and we expect the planet to undergo Type I migration. A typical
observed evolution outcome of such simulations is stopping of inward migration close to the tidally
truncated cavity. Once the planet has reached a quasistationary orbit, we allow gas accretion onto the core
and examine whether such a scenario can reasonably reproduce the observed systems. Removal of the gas disc
occurs in these simulations to mimick photoevaporation on a specified time scale.
4 Evolution of fullyformed planets
Here we examine the orbital evolution of embedded planets with masses corresponding to the observed values for the three systems Kepler16, Kepler34 and Kepler35. The aim is to investigate how the evolution depends on the employed disc model, and whether or not decent agreement with the observed planet parameters can be obtained.
4.1 Kepler16b
For our different isothermal disc models, the orbital evolution of an embedded planet with mass ratio corresponding to that of Kepler16b () is presented in the upper panel of Fig. 4. Using the gap opening criteria of Crida et al. (2006) which predicts that gap opening should occur provided that
(5) 
we expect an embedded circumbinary planet with mass ratio to significantly perturb the underlying surface density profile in the discs with , and . This is illustrated in the upper panel of Fig. 5 which displays the disc surface density profile at orbits for all disc models. Gap formation is clearly apparent in the case with , leading also to a substantial increase of the surface density in the inner disc. This results in a strong positive torque being exerted by the inner disc on the planet that prevents inward migration. This result is robust against the choice of inner boundary condition as we performed a simulation using a viscous outflow condition (see Pierens & Nelson 2008) and found no differences.
For disc models with , early evolution typically involves rapid inward migration due to the high surface density at the outer edge of the tidally truncated cavity. At later times the migration rate decreases as the planet enters the cavity and evolves in a region where the surface density gradient is positive. During the run with and inward migration stops with the planet settling into an orbit with eccentricity . Migration appears to stop due to the development of a strong positive corotation torque which counterbalances the Lindblad torque within the inner cavity where the surface density has a positive gradient (Masset et al. 2006a), as illustrated in the upper panel of Fig. 5. Saturation of the corotation torque can be prevented provided the viscous timescale across the horseshoe region , where is the halfwidth of the horseshoe region, is smaller than the horseshoe libration timescale . Equating these time scales yields an estimate of the minimum value for the viscous stress parameter, , required to avoid corotation torque saturation. We find:
(6) 
where we have used the fact that for , the halfwidth of the horseshoe region is (Masset et al. 2006b). For this gives , indicating that the corotation torque is indeed unsaturated for this model. In order to clearly demonstrate that this effect is at work here, we have followed the approach of Pierens & Nelson (2007) and computed semianalytically the torques experienced by the planet using the formulae in Paardekooper et al. (2011). The corotation, Lindblad and total torques exerted on the planet for the three models with and are presented as a function of the orbital radius in the lower panel of Fig. 5. Only in the model with and is the corotation torque seen to be larger than the Lindblad torque inside the cavity, giving rise to the location AU where the total torque cancels. Such a value is consistent with the simulation result that migration stops at AU.
For the two models with , and the corotation torque is much more saturated and the planet is expected to migrate inward further. Consistent with this prediction, the planet is observed to migrate all the way into the inner cavity in the simulation with . Due to the very long run times required by the simulations, the evolution outcome remains uncertain but the fact that there is a significant amount of gas within the cavity for this disc model (see upper right panel of Fig. 1) suggests that inward migration may proceed until the planet enters the region of dynamical instability located at AU. Extrapolating the observed migration rate forward in time, we estimate that the planet will migrate from AU to AU in yr, which is much smaller than the disc life time. An alternative outcome, however, may be capture in a mean motion resonance with the binary before dynamical instability occurs.
Contrary to the above prediction concerning saturation of the corotation torque, the run with and shows stalling of inward migration from P. This stalling does not arise because of a strong positive corotation torque, but rather because migration and gap formation by the planet, combined with tidal truncation by the binary, cause the disc material sitting between the planet and cavity to form a narrow ring. This increases the local surface density in the ring, giving a stronger positive contribution to the Lindblad torque experienced by the planet. This is illustrated in Fig. 6 which shows the evolution of the total torque experienced by the planet, and the contributions from the disc lying interior and exterior to the planet semimajor axis. As time proceeds the amplitude of the (positive) innerdisc torque increases while the (negative) outerdisc torque weakens and the planet halts when the inner and outer torque are in balance.
For the disc model with and , a similar process does not occur simply because the inner cavity is much deeper in that case. As can be shown in the upper panel of Fig. 5, the inner disc is completely depleted and the evolution outcome appears to be inward migration until the amount of local gas in the cavity becomes too small to make the planet migrate further in. For this model we have performed a long term evolution run for P and the results are presented in Fig. 7. At P, we see that inward migration is temporarily halted as the planet reaches AU. This corresponds to the location of the resonance with the binary. From this time the planet evolves for binary orbits without migrating just outside the resonance with its eccentricity oscillating between . At P the planet migrates inward through the 6:1 resonance and halts at semimajor axis close to the currently observed value ( AU). At the end of the simulation, the planet eccentricity oscillates between , while Kepler data gives .
4.2 Kepler34b
The middle panel of Fig. 4 shows the temporal evolution of the semimajor axis and eccentricity of a planet with , the mass ratio reported for Kepler34b. Eq. 5 suggests that a shallow gap can be formed in the calculation with , and in the one with and . Significant gap formation is not expected in the other runs.
The evolution is found to be unstable in the simulation with , with the planet experiencing a close encounter with the central binary at P. This is likely to arise because the disc is highly eccentric (as indicated by the left middle panel of Fig. 1), which drives a large planet eccentricity.
During the runs with and the planet migrates inward until the eccentricity increases to , at which point migration stalls due to torque reversal. A planet on a significantly eccentric orbit has smaller angular velocity at apocentre than neighbouring disc material, resulting in the outer disc exerting a positive torque on the planet. The opposite happens at pericentre and the inner disc exerts a negative torque. In general the total orbitaveraged torque experienced by a planet is expected to go from having negative to positive values as the eccentricity grows above values (Papaloizou & Larwood 2000). For a single planet embedded in a disc this does not normally imply that migration changes from being inward to outward because energy loss associated with eccentricity damping still causes the semimajor axis to decrease, albeit more slowly than for a circular orbit (Cresswell et al 2007). When the eccentricity is maintained through interaction with the central binary, however, then the total time averaged torque can equal zero and inward migration can be halted. In order to demonstrate that this effect is at work we follow Pierens & Nelson (2008) and plot the disc torque and the planet orbital position over a few planet orbital periods for the run with in Fig. 8. As expected, the torque exerted on the planet is positive (resp. negative) when the planet is at apocentre (resp. pericentre) and the orbitaveraged torque almost cancels. As noted by Pierens & Nelson (2008), the slight phase shift between the two curves is due to the time needed for the planet to create an inner (outer) wake at apocentre (pericentre). While Kepler34b is observed to orbit at AU from the central binary, we note that the final planet semimajor axis in the run with and is AU whereas it is AU in the calculation with . Interestingly, the final value for the eccentricity obtained in both runs is rather close from the observed value ().
For the two runs with (, ) and (, ) early evolution proceeds similarly, with the planet migrating inward until its eccentricity has increased to a value of , at which point migration stops. As mentioned above, however, the planet can significantly perturb the disc surface density profile in these two cases and this causes the planet to migrate inward at later times because the balance of torques is modified. In both cases the planet migrates inward again from binary orbits but the final outcome of each run differs. In the run the planet eccentricity decreases somewhat as the planet migrates deep inside the truncated cavity. Continuation of the run until binary orbits shows that migration eventually halts when the total orbitaveraged torque vanishes due to the finite eccentricity (see discussion above). At the end of the run the planet semimajor axis reaches a constant value AU and the eccentricity , much smaller than the observed eccentricity of Kepler34b. In the simulation with and significant growth of the planet eccentricity occurs at binary orbits, causing the planet to undergo an episode of outward migration. Analysis of this simulation shows that this sudden growth of is caused by interaction between the planet and an arcshaped high density structure related to the eccentric mode in the disc, with pattern speed of binary orbits. This is illustrated in the upper panel of Fig. 9 which shows a snapshot of the disc surface density at binary orbits. In the lower panel of Fig. 9, we plot the temporal evolution of the theoretical change of the planet eccentricity due to the disc with (e.g. Bitsch & Kley 2010):
(7) 
where is the estimated planet orbital decay rate, is the torque exerted by the disc on the planet and is the angular momentum of the planet. This figure clearly demonstrates that the disc is responsible for driving the planet eccentricity upward at . At later times it appears that the combined effect of eccentricity growth and outward migration cause the planet to be in contact with the disc density bump located at AU (see upper panel of Fig. 9), corresponding to material with higher specific angular momentum than the planet. Strong damping of the planet eccentricity occurs at and the planet migrates inward again. The longterm trend is of decreasing semimajor axis and eccentricity until the torque on the planet becomes negligible. At binary orbits the planet semimajor axis is AU and its eccentricity has reached a quasistationary value of , much smaller than the observed value (). The low value for arises because the planet orbits deep inside the tidallytruncated cavity where interaction with the eccentric disc is small. It is also related to the fact that for Kepler34, so that the forced eccentricity due to interaction with the binary is small. Continuation of this run for binary orbits confirms that the planet migrates very slowly into the gas depleted cavity on a nearcircular orbit, but too close to the central binary to be consistent with the observed orbital parameters of Kepler34b. At binary orbits, the planet semimajor axis is AU but there remains evidence that inward migration has not stalled completely.
4.3 Kepler35b
The orbital evolution of the Kepler35b simulations are shown for the different disc models in the lower panel of Fig. 4. Compared with Kepler34b, for which , the mass ratio of Kepler35b is . Despite the lower binary eccentricity the results for this system look rather similar to the corresponding Kepler34b runs.
For disc models with and the evolution outcomes are stalling of inward migration leaving the planet on an eccentric orbit at fixed semimajor axis. As we have seen in the previous section, this quasiequilibrium state is reached when the large positive torque experienced by the planet at apocentre is in exact balance with the weaker negative torque felt by the planet at pericentre. The final position of the planet is clearly correlated with the size of the tidally truncated inner cavity. For example, in the run with and , the density peak is located at AU (see lower right panel of Fig. 1) and the final planet semimajor axis is AU whereas in the simulation with and , the density peak is at AU and migration stops at AU. Not surprisingly, the final value for the planet eccentricity appears to scale with the disc eccentricity. For instance, in the run with and , the disc eccentricity is (see left panel of Fig. 1) and the final . In the run with , the disc eccentricity and at the end of the calculation.
A similar outcome is observed in the run with . Here the planet migrates rapidly inward at early times until it reaches a stable, nonmigrating configuration with AU and . Although not shown here, analysis of the torque experienced by the planet clearly reveals a positive (resp. negative) disc torque at planet apocentre (resp. pericentre) and a zero timeaveraged total torque.
For the simulation with and the process described above makes migration stall at binary orbits once the planet eccentricity has reached and its semimajor axis AU. Similarly to the case of Kepler34b, the planet is found to migrate inward again at later times due to gap formation by the planet. Subsequent evolution again corresponds to the planet migrating deep inside the inner cavity until the local disc mass becomes too small for further substantial migration. Despite a runtime of binary orbits, an equilibrium state was not reached for this case. At the end of the run, the planet semimajor axis is but inward migration still proceeds. Its eccentricity, however, has reached a constant value of . Again, such a low value for with respect to the observed one () arises because interaction betwen the planet and the eccentric disc is weak inside the cavity, and the binary mass ratio for Kepler35 so the forced eccentricity remains small.
5 Evolution of migrating and accreting protoplanets
We now consider a scenario in which a M core forms in the disc at large distance from the central binary and migrates inward via type I migration until it reaches a location where migration halts. For a M planet and for the fiducial value of the disc aspect ratio , the halfwidth of the horseshoe region is (Paardekooper et al. 2010), which means that at AU ( in the computational domain), the horseshoe region is resolved by about grid cells in the radial direction. For such a resolution, the relative error on the corotation torque is estimated to be (Masset 2002). Once migration is stalled, the planet then accretes gas from the disc until the disc has been dispersed by photoevaporation. The primary reason for including photoevaporation is that the planets in the Kepler16, Kepler34 and Kepler35 systems are Saturnian mass, and we know from calculations of giant planet formation that such planets are able to accrete gas at very rapid rates (e.g. Pollack et al 1996). It seems likely that Saturnmass planets embedded in a substantial reservoir of gas will grow rapidly, so we work with the assumption that growth beyond their observed masses was prevented by removal of the gas disc.
Our procedure is as follows. We first calculate the orbital evolution of protoplanets with mass ratio interacting with the different circumbinary disc models to illustrate the behaviour for different disc parameters. A typical outcome is stopping of inward migration close to the edge of the tidally truncated cavity, and this arises when the planet eccentricity reaches a value . For each of the Kepler binary systems we restart the simulation which uses the disc model that best reproduces the orbital parameters of the observed planet among the simulations presented in Sect. 4, switching on gas accretion onto the core. The final mass and orbital parameters of the planet are set by the gas dispersion timescale.
5.1 Evolution of a protoplanetary core
For the different isothermal disc models we consider, the orbital evolution of an embedded circumbinary protoplanet with mass ratio is presented in Fig. 10. The upper panel shows the results of simulations in which the binary parameters are those of Kepler16. The middle and lower panels correspond to the Kepler34 and Kepler35 systems.
We begin presentation of the simulation results by focusing on these two latter cases, for which similar outcomes are observed. Early evolution typically involves inward migration of the protoplanet and continued growth of its eccentricity due to its interaction with both the central binary and the eccentric disc. At later times inward migration slows down significantly in the run with , and completely stalls or even reverses for thinner disc models. In these cases the final location of the planet is clearly correlated with the position of the gap edge in the right panel of Fig. 1. For example, considering the Kepler34 system, the density peak is located at AU in the simulation with while the middle panel of Fig. 10 shows that migration stops at AU for the same disc model. In the fiducial run with and , the density peak is located at AU and the planet migrates to AU before migration halts. We plot both the surface density profile and the planet position at binary orbits in the upper panel of Fig. 11 for this run, showing that the planet halts at the edge of the cavity. As with a number of the simulations described in Sect. 3, the halting of migration occurs because of the torque reversal that occurs when . For eccentric orbits the corotation torque is expected to be substantially diminished (e.g. Bitsch & Kley 2010), so they cannot be responsible for the halting of migration. Following a strategy similar to that described in Sect. 4.2, where the correlation between the disc torque and the planet orbital radius is examined, we confirm that at late times the planet experiences a positive torque at apocentre and a negative torque at pericentre, leading to a null timeaveraged total torque. This is illustrated in the lower panel of Fig. 11 where we plot both the disc torque and the planet orbital position over a few orbital periods of the planet for the run with and .
The outward migration that we observe in simulations with and is likely related to the steepness of the inner cavity edge for these disc models, which combined with the fact that the planet spends more time at apocentre, favours a net positive torque on the planet. In runs with , however, the gradient of surface density in the inner cavity is shallower and so less favourable for stalling or reversing of migration for an eccentric planet. This explains why type I migration is not halted in that case.
The results of the Kepler16 runs are displayed in the upper panel of Fig. 10. Overall, these are consistent with the corresponding Kepler34 and Kepler35 simulations, except for the runs with (, ) and (, ) in which the final fate of the planet is found to be very different. In the simulation with , migration reverses at binary orbits due to the eccentric planet orbit, but outward migration accelerates from binary orbits onward. Inspection of the apsidal lines for both the disc and the planet reveals that from this time these become misaligned, with a tendency for the apsidal line of the disc to slightly lead that of the planet. This promotes outward migration because the planet interacts preferentially with matter whose angular velocity is greater than that of the planet at apocentre (Pierens & Nelson 2008). As outward migration proceeds, the planet eccentricity progressively decreases. Continuation of the run shows that the planet eventually migrates inward again once its semimajor axis has reached AU. Therefore we can reasonably expect the long term evolution for this run to consist of periods of inward followed by outward migration until disc dispersal.
With respect to the other disc models, the positive gradient of surface density at the inner edge of the tidally truncated cavity is shallower in the simulation with (, ) (see upper right panel of Fig. 1). Consequently, torque reversal is not observed in that case and the planet migrates inward continuously. This inward migration is accompanied by significant growth of the planet eccentricity due to its interaction with both the binary and eccentric disc. The eccentricity increases to at P. At , the eccentricity growth causes the planet to undergo a close encounter with the binary and to be subsequently ejected from the system.
5.2 Evolution of an accreting core
In this section we use the disc model that best reproduces the observed parameters of each of the three Kepler systems to focus on a more realistic evolution scenario in which a migrating embryo grows by accreting gas from the disc at the same time as the disc is being dispersed. We expect both core growth and inward migration to be terminated as a result of disc clearing, which is thought to be mainly driven by photoevaporation induced by UV irradiation and/or Xrays at late times (Owen et al. 2011). Gas disc dispersal by photoevaporation is modelled in the simplest possible manner by forcing the gas surface density to decay exponentially with an efolding time , for which we consider values and P. These values are broadly consistent with estimates of the gas dispersal timescale due to UV photoevaporation which give years (Alexander et al. 2006). We also vary the rate at which the planet accretes gas from the disc by choosing different values for the accretion parameter, , defined in Sect. 2.2. For each value of disc dispersal time we perform simulations for values of , 2, 3, …, 10. We note that corresponds to the maximally accreting planet (e.g. Kley 1999).
Kepler16
A core mass of is close to the value required for runaway gas accretion in the core accretion scenario of gas giant planet formation (Pollack et al. 1996; Papaloizou & Nelson 2005), which is why this core mass was chosen for these simulations. The disc model that gave best agreement with the observed orbital parameters of Kepler16b in Sect. 4.1 had and , so we consider a model that was run with planetary mass ratio () until migration halts, and then restart with gas accretion and photoevaporation switched on for the model parameters described above.
The evolution of the model that best fits the observed Kepler16b system is shown in the top panels of Fig. 12, and had parameters and P. The left panel shows the planet and disc masses, and the right panel shows the semimajor axis and eccentricity. The planet mass slightly exceeds the inferred mass of Kepler16b, the semimajor axis stalls just outside of the observed value, and the eccentricity has a mean value (to be compared with the smaller value of inferred from observations). It seems very likely that subtle tweaking of the model parameters could lead to a planet whose mass and semimajor axis agrees much more accurately with the observed values, but our aim here is not to obtain perfect agreement with the observed values using a highlysimplified disc model so we do not attempt to refine the values of and here. Obtaining a mean eccentricity equal to the very small value reported for this system would appear to present a greater challenge. It remains to be seen whether a more realistic disc model will lead to a smaller final planet eccentricity.
Kepler34
The simulations in Sect. 4.2 indicate that the disc parameters and best produce a final planetary configuration that approximates the observed values. The simulation with planetary mass ratio described in Sect. 5.1 above was restarted with gas accretion and disc dispersal switched on, and the results from the run whose outcome best matches the observed Kepler34b system are shown in the middle panels of Fig. 12. This simulation adopted and P. We see that the simulated planet mass undershoots the observed value slightly (a slightly larger value of would presumably improve this). We see that the semimajor axes and eccentricities barely change at all during the time when gas accretion occurs, suggesting that the final orbital configuration obtained for the 20 M embryo is very similar to that for the final planet after accretion. Inspection of Fig. 4 shows that migration of the fullyformed planet also leads to very similar final values for and . Unlike in the Kepler16 run, the simulations of Kepler34b using the disc model and produce the same set of orbital elements when considering a fullyformed planet, a migrating 20 M core, and a gasaccreting core. Producing a closer approximation to the observed system will therefore require modest tweaking of the disc physics rather than the parameters and .
Kepler35
The disc model with and was shown to be the best candidate for reproducing the orbital configuration of Kepler35b in Sect. 4.3. The simulation with planetary mass ratio described in Sect. 5.1 above was restarted with gas accretion and disc dispersal switched on, and the results from the run whose outcome best matches the observed Kepler35b system are shown in the lower panels of Fig. 12. This simulation adopted and P, and produces a planet mass close to the one observed, but a semimajor axis that is larger than the observed value ( AU versus 0.6 AU). This is consistent with the corresponding run with the fully formed planet in Sect. 4.3 which also resulted in a planet with . Reducing this value to agree with the observed one will therefore require moderate adjustment of the disc model. The eccentricity evolution results in a final mean value of . Interestingly this is smaller than the observed value of 0.04, unlike the value obtained from the simulation of the fullyformed planet which resulted in (see Fig. 4).
It is clear from this and the other simulations described for Kepler35b and Kepler16b that obtaining fits to the observations for all system parameters would require implementation of a multidimensional fitting procedure whose complexity would not be justified given the simplicity of our underlying model.
5.3 Validity of the isothermal approximation
In the locally isothermal limit, the only contribution to the corotation torque is the vorticityrelated
corotation torque which scales with the vortensity (i.e. the ratio between vorticity and
surface density) gradient. In the context of circumbinary discs, it has been shown that at the inner edge of the tidally truncated cavity where the surface density has
a large positive gradient, the (positive) vorticityrelated corotation torque can be strong enough to
counterbalance the (negative) differential Lindblad torque, leading to halting of Type I migration
(Masset et al. 2006; Pierens & Nelson 2007). This arises provided that the amplitude of the corotation torque is
close to its optimal value, which is reached when: i) the viscous diffusion
timescales across the horseshoe region are approximately equal to half the libration timescale (Baruteau & Masset 2013); ii) the planet eccentricity
is significantly smaller than the dimensionless halfwidth of the horseshoe region . We expect indeed that when , the radial
excursion of the planet becomes larger than the halfwidth of the horseshoe region and consequently the corotation
torque to be strongly attenuated (Bitsch & Kley 2010).
For , which is a value typical to what is observed in the isothermal simulations of cores presented
above,
it is likely that the contribution of the corotation torque to the total torque is relatively weak
(see Fig. 2 of Bitsch & Kley 2010).
In nonisothermal discs, the corotation torque consists of the vorticityrelated corotation torque
plus an additional component which scales with the entropy gradient (Paardekooper & Papaloizou 2008;
Baruteau & Masset 2008). For a negative entropy gradient inside the disc, this entropyrelated corotation
torque is positive and can be responsible for significantly slowing down or even reverse Type I migration. Depending on
whether or not a locally isothermal equation of state is used and provided that the amplitude of the corotation
torque is close to its fullyunsaturated value, simulations of the evolution of cores in the Kepler16, Kepler34 and Kepler35 systems may therefore lead to very different outcomes. Regarding the simulations with fullyformed
planets, we note that the issue of the equation of state does not really matter since we expect a Saturnmass planet
to open a partial gap in the disc, with the consequence that the corotation torque is weakened (Kley & Crida 2008).
Assuming a core forming at AU (Marzari et al. 2013), namely in a region of small
disc eccentricity, its migration can
be directed
either outward or inward in the nonisothermal case, depending on the level of saturation of the corotation torque. In both cases, however, we expect
the protoplanet to reach a zeromigration line where it becomes trapped (Lyra et al. 2010; Hellary & Nelson 2012). As the disc disperses,
the zeromigration line is shifted inward with the main consequence that the planet eventually enters a region of high disc eccentricity. In that case, the
embryo should decouple from the zeromigration line at a point in time where its eccentricity becomes high enough
for the corotation torque to be significantly weakened. The planet then migrates inward again and
we expect evolution outcomes rather similar to those arising in isothermal runs. This implies that in the phase
after the embryos eccentricities have reached values , the results of
isothermal runs presented above are relatively robust regarding the equation of state.
In disc models with moderate values
of disc eccentricity, if any, an alternative outcome is that the planet moves inward as the disc disperses until it reaches
the inner edge of the inner cavity where it becomes trapped due to the action of the vorticityrelated corotation
torque.
As the planet eccentricity is mainly driven by the eccentric disc, this raises the issue of the disc eccentricity in the radiative case. Clearly, this issue needs to be examined in more details
and we will address this issue and its consequence on the evolution of protoplanetary cores in the Kepler16,
Kepler34 and Kepler35 systems in a future publication.
6 Discussion and conclusion
In this paper, we have presented the results of hydrodynamic simulations that examine the migration and orbital evolution of embedded circumbinary planets orbiting around the three close binary systems Kepler16, Kepler34 and Kepler35. We began our study by examining the evolution of the binaryplusdisc system in the absence of an embedded planet in order to obtain an improved understanding of how circumbinary discs are structured by the central binary as a function of binary and disc parameters. In particular, we examined how the mean surface density radial profile and disc eccentricity vary for the three Kepler binary systems as a function of disc aspect ratio, , and viscosity parameter . Our results indicate that for each binary system the disc structure is a sensitive function of the disc parameters, with the tidally trucated cavity displaying significant changes in both radius and internal density structure as a function of and . Furthermore, the eccentricity of the disc also shows strong dependence on disc parameters: we observe a general tendency for the disc eccentricity to increase with increasing , which is likely due to the fact that the eccentricity is more effectively communicated through the disc for larger values of .
Our investigation confirms that the origin of the disc eccentricity is non linear mode coupling as described previously for circumbinary and circumstellar discs by Papaloizou et. al. (2001) and Lubow (1991), respectively. The forced eccentricity due to secular interaction with the binary is too small to explain the simulations (see Sect. 3.1). The Papaloizou et al (2001) study indicated that coupling between an initial eccentric disc disturbance and the component of the binary potential with pattern speed equal to the mean motion of the binary leads to excitation of a wave at the 3:1 eccentric Lindblad resonance which transports angular momentum outward, increasing the disc eccentricity. Our study indicates that the 3:1 resonance is important also for the eccentric Kepler binary systems, but also suggests that mode coupling involving higher order terms in the binary potential may also be important. Given the importance of the disc eccentricity for determining the orbital parameters of embedded circumbinary planets, a further, more indepth study of circumbinary disc dynamics is certainly warranted.
Our study of the evolution of circumbinary planets embedded in the circumbinary discs described above adopted two basic scenarios. In the first we considered the orbital evolution of a fullyformed planet in a variety of disc models for each binary system, and attempted to determine which of the disc models resulted in planet orbits that best agree with the Kepler observations. The basic mode of evolution in these runs was inward migration of the planet, followed by stalling of migration in the tidally truncated disc cavity. The planetary orbits typically become noncircular due to interaction with the circumbinary disc and binary, with the former effect usually being dominant. In the second, more realistic scenario, we consider the evolution of a lowmass ( M) core, which migrates inward until it stalls when it enters the inner disc cavity. Gas accretion onto this core is then initiated, along with dispersal of the gas disc (mimicking photoevaporation for example), until the planet achieves its final mass and orbital configuration. We examine the outcome of this scenario as a function of gas accretion rate onto the planet and disc dispersal time scale, and for each of the Kepler binary systems we form circumbinary planets which are similar to the observed systems. Furthermore, we generally find that for each of the Kepler binary systems the final orbital configuration of the planet is similar, independent of the two migration scenarios adopted (fullyformed planet versus migrating and accreting core).
We find that the simulation that produces the closest approximation to the observed system for each of the Kepler binaries uses a different disc model: no single disc model produces a final planet that is in close agreement with the observational data for all planets. For Kepler16b, a disc model with and produces the bestfit. Good agreement with the observed planet mass and semimajor axis can be obtained, but all models consistently predict a larger eccentricity for the planet than observed (typically is obtained, compared with the observed value of ). Given that the eccentric disc is largely responsible for the eccentricity growth, this indicates that a model with smaller disc eccentricity may be required to provide a better fit. For Kepler34b the disc with and best reproduces the orbital parameters of the planet. For this system a plausible model of core formation at large radius followed by inward migration and gas accretion can be constructed that provides a good fit to the planet mass and eccentricity, but none of our simulations were successful in forming a planet whose final semimajor axis is as small as observed (values of AU were obtained, to be compared with the observed value of 1.1 AU). The stalling of migration occurs through an interplay between the planetary eccentricity and the surface density profile in the inner cavity, since this is what determines the averaged torque balance. Obtaining the required surface density profile very likely requires a more sophisticated disc model in which either or are not constant. For Kepler35b a disc model with and produces the best fit to the planet orbital parameters. A simple model of core migration followed by gas accretion and disc dispersal can form a planet with mass close to the observed value, but in general the semimajor axis stalls at a value that is too large (values of AU are obtained, compared with the observed value 0.6 AU). The bestfit migrationplusaccretion model for this system produces an eccentricity that is too small (in stark contrast to the Kepler16b runs), with a mean value of being obtained, versus the observed value of 0.04. Interestingly, the bestfit model for a fullyformed planet that migrates in and stalls produces a value , so the observed value falls neatly between these two simulated values. Again, it is likely that the details of the disc eccentricity distribution and the surface density profile in the inner disc cavity determine the fine details of the planetary orbital parameters, and obtaining improved fits may simply require a more sophisticated disc model than we have considered.
In summary, our simulation results indicate strongly that the Kepler16, Kepler34 and Kepler35 planets can be explained by a scenario in which a massive rocky/icy core forms at large distance from the central binary in a circumbinary disc and migrates inward until it stalls in the tidally truncated cavity formed by the central binary. Subsequent gas accretion leads to the growth of the planet, and the changing balance of torques leads to a further episode of modest inward migration. We argue that the final configurations of these planets are likely to be determined in part by dispersal of the gas disc, since the observed planets are all expected to be in the regime where runaway gas accretion can occur (e.g. Pollack et al 1996; Papaloizou & Nelson 2005) – i.e. in the saturnian or subsaturnian mass range.
The models we have presented are in essence the simplest we can compute, so our intention has not been to provide rigorous fits to the observational data. Instead, our aim was to demonstrate the plausibility of the core formation, migration and gas accretion picture for each of the Kepler circumbinary planets. Our simulations demonstrate the importance of the circumbinary disc structure for determining the final parameters of forming circumbinary planets, and it is clear that improved understanding of these systems will require more indepth modelling that includes radiation transport, selfgravity and additional processes that determine the detailed stucture of the circumbinary disc. These issues will be examined in a future publication.
Acknowledgements.
Computer time for this study was provided by the computing facilities MCIA (Mésocentre de Calcul Intensif Aquitain) of the Université de Bordeaux and by HPC resources from GENCIcines (c2012046957).References
 Alexander, R. D., Clarke, C. J., & Pringle, J. E. 2006, MNRAS, 369, 229
 Artymowicz, P., & Lubow, S. H. 1994, ApJ, 421, 651
 Baruteau, C., & Masset, F. 2008, ApJ, 672, 1054
 Baruteau, C., & Masset, F. 2013, Lecture Notes in Physics, Berlin Springer Verlag, 861, 201
 Bell, K. R., & Lin, D. N. C. 1994, ApJ, 427, 987
 Binney, J., & Tremaine, S. 1987, Princeton, NJ, Princeton University Press, 1987, 747 p.,
 Bitsch, B., & Kley, W. 2010, A&A, 523, A30
 Cresswell, P., Dirksen, G., Kley, W., & Nelson, R. P. 2007, A&A, 473, 329
 Crida, A., Morbidelli, A., & Masset, F. 2006, Icarus, 181, 587
 Crida, A., Baruteau, C., Kley, W., & Masset, F. 2009, A&A, 502, 679
 de ValBorro, M., Edgar, R. G., Artymowicz, P., et al. 2006, MNRAS, 370, 529
 Doyle, L. R., Carter, J. A., Fabrycky, D. C., et al. 2011, Science, 333, 1602
 Dutrey, A., Guilloteau, S., & Simon, M. 1994, A&A, 286, 149
 Günther, R., Schäfer, C., & Kley, W. 2004, A&A, 423, 559
 Hellary, P., & Nelson, R. P. 2012, MNRAS, 419, 2737
 Holman, M. J., & Wiegert, P. A. 1999, AJ, 117, 621
 Hubeny, I. 1990, ApJ, 351, 632
 Kley, W. 1999, MNRAS, 303, 696
 Kley, W., & Nelson, R. P. 2010, Astrophysics and Space Science Library, 366, 135
 Lin, D. N. C., & Papaloizou, J. 1986, ApJ, 309, 846
 Lubow, S. H. 1991, ApJ, 381, 259
 Lyra, W., Paardekooper, S.J., & Mac Low, M.M. 2010, ApJ, 715, L68
 Masset, F. 2000, A&AS, 141, 165
 Masset, F. S., D’Angelo, G., & Kley, W. 2006, ApJ, 652, 730
 Masset, F. S., Morbidelli, A., Crida, A., & Ferreira, J. 2006, ApJ, 642, 478
 Marzari, F., Thébault, P., & Scholl, H. 2008, ApJ, 681, 1599
 Marzari, F., Scholl, H., Thébault, P., & Baruteau, C. 2009, A&A, 508, 1493
 Marzari, F., Baruteau, C., Scholl, H., & Thebault, P. 2012, A&A, 539, A98
 Marzari, F., Thebault, P., Scholl, H., Picogna, G., & Baruteau, C. 2013, A&A, 553, A71
 Meschiari, S. 2012, ApJ, 752, 71
 Meschiari, S. 2012, ApJ, 761, L7
 Moriwaki, K., & Nakagawa, Y. 2004, ApJ, 609, 1065
 Nelson, R. P., Papaloizou, J. C. B., Masset, F., & Kley, W. 2000, MNRAS, 318, 18
 Nelson, R. P. 2003, MNRAS, 345, 233
 Orosz, J. A., Welsh, W. F., Carter, J. A., et al. 2012, ApJ, 758, 87
 Orosz, J. A., Welsh, W. F., Carter, J. A., et al. 2012, Science, 337, 1511
 Owen, J. E., Ercolano, B., & Clarke, C. J. 2011, MNRAS, 412, 13
 Paardekooper, S.J., & Papaloizou, J. C. B. 2008, A&A, 485, 877
 Paardekooper, S.J., Baruteau, C., Crida, A., & Kley, W. 2010, MNRAS, 401, 1950
 Paardekooper, S.J., Baruteau, C., & Kley, W. 2011, MNRAS, 410, 293
 Paardekooper, S.J., Leinhardt, Z. M., Thébault, P., & Baruteau, C. 2012, ApJ, 754, L16
 Papaloizou, J. C. B., & Larwood, J. D. 2000, MNRAS, 315, 823
 Papaloizou, J. C. B., Nelson, R. P., & Masset, F. 2001, A&A, 366, 263
 Papaloizou, J. C. B., & Nelson, R. P. 2005, A&A, 433, 247
 Pelupessy, F. I., & Portegies Zwart, S. 2013, MNRAS, 429, 895
 Pierens, A., & Nelson, R. P. 2007, A&A, 472, 993
 Pierens, A., & Nelson, R. P. 2008, A&A, 478, 939
 Pierens, A., & Nelson, R. P. 2008, A&A, 483, 633
 Pollack, J. B., Hubickyj, O., Bodenheimer, P., et al. 1996, Icarus, 124, 62
 Press, W. H., Teukolsky, S. A., Vetterling, W. T., & Flannery, B. P. 1992, Cambridge: University Press, —c1992, 2nd ed.,
 Scholl, H., Marzari, F., & Thébault, P. 2007, MNRAS, 380, 1119
 Schwamb, M. E., Orosz, J. A., Carter, J. A., et al. 2013, ApJ, 768, 127
 Shakura, N. I., & Sunyaev, R. A. 1973, A&A, 24, 337
 Tanaka, H., Takeuchi, T., & Ward, W. R. 2002, ApJ, 565, 1257
 van Leer, B. 1977, Journal of Computational Physics, 23, 276
 Ward, W. R. 1997, Icarus, 126, 261
 Welsh, W. F., Orosz, J. A., Carter, J. A., et al. 2012, Nature, 481, 475
 Winn, J. N., Albrecht, S., Johnson, J. A., et al. 2011, ApJ, 741, L1