Gravitational Wave Signatures of Ab Initio Two-Dimensional Core Collapse Supernova Explosion Models for 12-25 Solar Masses Stars
We present the gravitational waveforms computed in ab initio two-dimensional core collapse supernova models evolved with the Chimera code for progenitor masses between 12 and 25 M. All models employ multi-frequency neutrino transport in the ray-by-ray approximation, state-of-the-art weak interaction physics, relativistic transport corrections such as the gravitational redshift of neutrinos, two-dimensional hydrodynamics with the commensurate relativistic corrections, Newtonian self-gravity with a general relativistic monopole correction, and the Lattimer–Swesty equation of state with 220 MeV compressibility, and begin with the most recent Woosley–Heger nonrotating progenitors in this mass range. All of our models exhibit robust explosions. Therefore, our waveforms capture all stages of supernova development: 1) a relatively short and weak prompt signal, 2) a quiescent stage, 3) a strong signal due to convection and SASI activity, 4) termination of active accretion onto the proto-neutron star, and 5) a slowly increasing tail that reaches a saturation value. Fourier decomposition shows that the gravitational wave signals we predict should be observable by AdvLIGO for Galactic events across the range of progenitors considered here. The fundamental limitation of these models is in their imposition of axisymmetry. Further progress will require counterpart three-dimensional models, which are underway.
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Core collapse supernovae (CCSNe) are recognized as the most energetic explosions in the modern Universe. As a result of the collapse and the subsequent explosion of a massive star (), gravitational binding energy of the progenitor ( ergs) is released in the form of neutrino radiation (%) and the kinetic energy of ejected material observed in the electromagnetic spectrum (%). Post-collapse asymmetries in fluid motion along with anisotropic emission of neutrinos also generate a strong burst of gravitational waves (GWs). The presence of three different types of radiation associated with CCSNe makes them ideal objects for multi-messenger astronomy Ando et al. (2013). Simultaneous observations of the multi-messengers from CCSNe can reveal not only the details of the supernova mechanism Logue et al. (2012) but also may shed light on fundamental properties of neutrinos Mosquera Cuesta and Lambiase (2008). Gravitational radiation signals are particularly interesting among them because they are the only signals that provide deep insight into the multidimensional dynamics of the supernova core. The uniqueness of the information carried by GWs was recognized quite early (for comprehensive reviews of GWs from CCSNe, see Kotake et al. (2007); Ott (2009); Kotake (2013)).
However, CCSNe are extremely complex and physically diverse phenomena that involve an intricate interplay of general relativistic gravity, hydrodynamics, and neutrino transport, and thermonuclear kinetics, on short time scales. The complexity of the problem requires state-of-the-art numerical simulations for a quantitative analysis of the processes taking place in the supernova core. This is a great challenge in and of itself. It is currently known that realistic simulations of CCSNe are multidimensional and include hydrodynamics, self-gravity, and neutrino transport with the complete set of neutrino weak interactions, preferably in full general relativity but with at least approximate general relativistic corrections to all three. Recent simulations of other groups that have provided gravitational waveforms met some of these requirements Murphy et al. (2009); Müller et al. (2013); Ott et al. (2013); Kuroda et al. (2014).
The first simulations of GW emission from core collapse supernovae were limited to rapidly rotating stellar core collapse Zwerger and Müller (1997); Dimmelmeier et al. (2002); Kotake et al. (2003); Ott et al. (2004). These simulations did not require a large amount of computational resources in order to produce the strongest part of the GW signal at bounce and, therefore, their primary waveforms are of relatively short duration (30–50 ms). More recent predictions of the signal from rapidly rotating collapsing cores Ott et al. (2007); Dimmelmeier et al. (2007, 2008); Kotake et al. (2009); Abdikamalov et al. (2010); Kotake et al. (2011); Takiwaki and Kotake (2011); Ott et al. (2012, 2013); Abdikamalov et al. (2014); Kuroda et al. (2014); Fuller et al. (2015) use two- or three-dimensional simulations, conformally-flat or full general relativity, along with, in some cases, a deleptonization prescription for the stellar core, developed to reproduce the results of a full neutrino transport treatment during the collapse phase Liebendörfer (2005) and a neutrino leakage scheme for the post-bounce evolution Ott et al. (2012). For the relatively short simulation time associated with these models, this approach is quite adequate. However, most supernova cores likely do not rotate rapidly Heger et al. (2005) to produce a strong GW signal.
Another class of CCSN simulations has focused on the GW signatures of hydrodynamic instabilities in the post-bounce phases – in particular, convection inside the proto-neutron star (PNS), neutrino-driven convection in the post-shock region Bethe (1990); Herant et al. (1994); Burrows et al. (1995); Janka and Müller (1996); Müller and Janka (1997), and the standing accretion shock instability (SASI) Blondin et al. (2003); Blondin and Mezzacappa (2006); Ohnishi et al. (2006); Foglizzo et al. (2007); Scheck et al. (2008); Iwakami et al. (2009); Fernández (2010). These models require that we simulate at least several hundred milliseconds of post-bounce time during which time all instabilities develop and achieve their nonlinear state, and potentially saturate, and during which time explosion also develops. In this case, a far more realistic treatment of neutrino transport is crucial. Although there has been recent significant progress (e.g., see Kuroda et al. (2015)), multidimensional CCSN models with realistic neutrino transport and full general relativity are not yet available. This is in part due to the shear computational cost associated with such models that cannot be paid on present-day supercomputing platforms. There are a few methods widely used to approximate neutrino transport in two- or three-dimensional models that do not require as much computational power: a parameterized approximation for neutrino heating and cooling Müller and Janka (1997); Kotake et al. (2007); Murphy et al. (2009); Kotake et al. (2009), gray neutrino transport schemes Fryer and Warren (2004); Müller et al. (2013), the IDSA method Scheidegger et al. (2010), and finally, but most notably, multi-group neutrino transport (e.g., multi-group flux-limited diffusion) in the “ray-by-ray-plus” approximation Buras et al. (2006). Previous studies Murphy et al. (2009); Marek et al. (2009); Yakunin et al. (2010); Müller et al. (2013) using one of these methods have established the fundamental structure of the waveform, which consists of three major components: a prompt-convection signal that lasts about 70 ms; the strongest part of the signal, due to neutrino-driven convection and the SASI (200 ms); and a signal due to the revived shock’s expansion, which produces a growing offset in GW amplitude. Uniqueness of the “ray-by-ray” method is that it allows us to estimate the contribution of anisotropic neutrino emission to the total GW signal Müller et al. (2004); Marek et al. (2009); Yakunin et al. (2010); Müller et al. (2013).
In this paper, we present the gravitational waveforms from four non-rotating axisymmetric (two-dimensional) relativistic models evolved with the neutrino-hydrodynamics code Chimera beyond one second of post-bounce time and explosion. We compare our results with both GW predictions from our previous simulations (A-series) Yakunin et al. (2010) and the results of other groups Müller et al. (2013); Ott et al. (2013). We discuss all of the features of the GW signals from the four models initiated from four different progenitors with masses 12, 15, 20, and 25 M. All of our waveforms are available for download from ChimeraSN.org.
Our paper is organized as follows. A brief description of the code and the model setup is given in Section 2. In Section 3, we describe the methods used for extraction and analysis of the GW signals. In Section 4, we provide gravitational waveforms for all of our models and the results of our analysis. In Section 5, we summarize our investigation and draw conclusions.
Ii Code Description and Model Setup
We analyze the GW emission in four two-dimensional simulations performed with the neutrino-hydrodynamics code Chimera Bruenn et al. (2014) . Chimera consists of five major modules: hydrodynamics, neutrino transport, self-gravity, a nuclear equation of state, and a nuclear reaction network.
Chimera solves the equations of Newtonian hydrodynamics but takes into account some effects of strong-field gravity by means of an “effective potential” Rampp and Janka (2002); Marek et al. (2006). The gravitational field is computed by multipole expansion Müller and Steinmetz (1995). We replace the Newtonian monopole component with a GR monopole Marek et al. (2006). It has been shown by Müller et al. (2010) that this approximation works very well for slow rotation. The neutrino transport module solves the energy-dependent neutrino moment equations for all neutrino flavors using an updated version of multi-group flux-limited diffusion (in the ray-by-ray-plus approach of Buras et al. (2006)) with a flux limiter that has been tuned to reproduce Boltzmann transport results Liebendörfer et al. (2004). The ray-by-ray-plus method is able to produce angular variations in the neutrino radiation field, which, in turn, generates low frequency GW signals (Figure 1).
In total, we evolve four different non-rotating, non-perturbed, axisymmetric models (designated B12-WH07, B15- WH07, B20-WH07, and B25-WH07, corresponding to zero-age main sequence progenitors of 12, 15, 20, and 25 M Woosley and Heger (2007)) on a spherical-polar mesh consisting of 512 non-equally-spaced, adaptive radial zones and 256 uniformly-spaced angular zones. In radius, the grid covers , , , and km, respectively. In angle, the grid goes from 0 to .
All presented models were simulated using the Lattimer–Swesty Lattimer and Swesty (1991) equation of state (EoS) with a bulk incompressibility modulus MeV for , which is capable of supporting the maximum observed neutron star masses of 2 M Demorest et al. (2010); Antoniadis et al. (2013), and an enhanced version of the Cooperstein EoS Cooperstein (1985) for where nuclear statistical equilibrium (NSE) applies.
All four progenitors are evolved beyond 1 second after core bounce. All models exhibit shock revival and the development of neutrino-driven explosions. The evolution beyond 1 second captures all important phases of the supernova dynamics that pronounce in the GW signals. Three of the models developed clear prolate shock morphologies, while the 20 M model develops an approximately spherical, off-center shock as the explosion begins, and then becomes moderately prolate at 600 ms after bounce. The morphologies of the explosions are reflected in the gravitational waveforms. The explosion geometry of the 20 M model has reduced not only the model’s explosion energy relative to the 15 and 25 M models but also the total energy emitted in the form of GWs.
Iii Gravitational Wave Extraction
We consider the slow-motion, weak-field approximation for post-processing extraction of the GW signal from our simulations.
iii.1 GWs Produced by a Time-Dependent, Mass-Quadrupole Moment
We consider only the lowest order terms in the retarded expansion of the mass-quadrupole formula Epstein (1975). The transverse-traceless part (TT) of the gravitational strain is given by
where is the distance from the source to the observer and the mass quadrupole is defined as
Here is the -component of the linearized stress-energy tensor
Optimal design of gravitational wave detectors requires some knowledge of the expected waveforms, the corresponding frequency spectra, and the total energy emitted by possible sources Hawking and Israel (1987). Thus, any extraction method should decrease the numerical noise as much as possible. Most numerical differentiation methods amplify the numerical noise built into the simulation data. To avoid this, is usually computed by reducing the order of time derivatives of :
Following Nakamura and Oohara (1989); Blanchet et al. (1990) and Finn and Evans (1990), the quadrupole signal can be expressed in terms of a volume integral depending only on the density, velocity, and the gradient of the gravitational potential:
Using the continuity equation in the integrand in Eq. (5), one can replace the density time derivative. Integrating by parts and omitting the surface contribution, we find the resulting integrand
where , and are the spherical coordinates in the source frame (-frame), is the component of velocity in the same frame.
Further reduction of the time derivative is conventionally done by using the momentum equation Nakamura and Oohara (1989); Blanchet et al. (1990). However, this has to be carried out carefully. The Euler equation includes stress terms. Therefore, in order to replace with balancing stress terms, we need to take into consideration all possible contributions to the stress terms, such as pressure, gravity, anisotropic neutrino forces acting on the fluid, effective viscosity that may present in the finite differencing of the momentum equation, etc. To avoid this issue, we have decided to compute for all time steps and to numerically evaluate to obtain . Numerical algorithms for computing first-order derivatives introduce far less numerical noise than those for higher-order derivatives. In order to determine the detectability of the GWs, we calculate the characteristic GW strain for a given frequency Flanagan and Hughes (1998) using
where is the GW energy spectrum and denotes the Fourier transform of :
The stochastic nature of GW signals from CCSNe prompts the use of short-time Fourier transform (STFT) techniques to determine the frequency of a signal as it changes over time Murphy et al. (2009):
where is the Hann window function Blackman and Tukey (1959).
iii.2 Gravitational Waves Produced by Anisotropic Neutrino Emission
Besides aspherical mass motion, any other sources with non-zero quadrupole moments will produce GW emission. One of these sources is the anisotropic radiation of neutrinos from the hot PNS. The theoretical derivation of the GW signal produced by a distant anisotropic point source of neutrinos was first published by Epstein (1978). Müller end Janka Müller and Janka (1997) were the first authors to implement this formalism. Kotake et al. (2007) improved the formalism and made it more suitable for numerical evaluation of GW signals.
The transverse-traceless part of the gravitational strain, , from neutrinos is given by Müller and Janka (1997)
Here is the solid angle in the -frame, and the vector is the direction of neutrino emission whose components are given with respect to the -frame. The tensor is the transverse-traceless part of the second-rank symmetric tensor with respect to the observer’s -axis (the -direction is defined as the direction connecting the source and the observer). The angles and define the direction of neutrino emission with respect to the -frame. The other factor in the integrand, , is the “direction-dependent neutrino luminosity” given in the -frame.
In the case of axisymmetry, both and components of the gravitational wave signal vanish for an observer on the symmetry axis, and the GW signal with the maximum amplitude will be detected by an observer in the equatorial plane Müller and Janka (1997). For such an observer, the gravitational strain is given by
Since our models are axisymmetric, we can simplify . Integrating over Kotake et al. (2007):
Iv Waveform Analysis
Gravitational waveforms covering all phases of GW emission and based on non-parameterized supernova explosions were first reported in the work of Yakunin et al. (2010). Here we present waveforms obtained in a new series of supernova simulations performed by our group Bruenn et al. (2013), and a comparison with our previous results.
iv.1 Qualitative Description of the GW Signals
GW signals from both matter and neutrino sources for the models B12-WH07, B15-WH07, B20-WH07, and B25-WH07 are provided in the left panels of Figure 1, and the evolution of the signal frequency is given in the right panels of the same figure. Qualitatively, our gravitational waveforms have all of the key features of waveforms described in previous studies of CCSNe based on models that explode Marek et al. (2009); Murphy et al. (2009); Yakunin et al. (2010); Müller et al. (2013). The GW signal passes through four distinct phases: 1) A prompt signal: an initial and relatively weak signal that starts at bounce and ends at about 80 ms post-bounce. 2) A quiescent stage that immediately follows the prompt signal and ends somewhere about 125 ms after bounce. 3) A strong signal, which follows the quiescent stage and is the most energetic part of the GW signal. This stage ends somewhere between 350 ms and 400 ms after bounce. 4) A “tail,” which starts just before the end of the strong phase, at about 300 ms after bounce and consists of a low-frequency component with increasing amplitude. This “tail” tends to rise during the simulations, but not monotonically. The signal produced by anisotropic neutrino emission exhibits a low-frequency “tail”-like behavior during the entire simulation.
The frequency evolution in Figure 1 shows how the characteristic frequency of the signal changes during the simulation. The initial frequency 500 Hz of the early signal drops to 100–200 Hz (the quiescent stage). The strong phase of the signal is characterized by a steady increase of the peak frequency, which reaches its maximum value of 700–800 Hz at 500–600 ms. Then, the frequency slowly decreases during the “tail” phase.
iv.2 Early Signal
The early GW signal is produced by entropy-driven convection in the PNS during the first 10 ms after bounce. Unlike in our previously published models (the “A-series”) Yakunin et al. (2010), in the models presented here (the “B-series”)Bruenn et al. (2013) we do not observe the high-amplitude, low-frequency contribution to the prompt signal due to the deflection of infalling matter through the shock. As a result, the peak amplitudes of the prompt signals in all the B-models decrease by a factor of 2–4 relative to their values in the corresponding A-series models (see the insets of Figure 2).
The results presented here are in agreement with the conclusions drawn by Müller et al. (2013), who estimated the contribution at the shock in their semi-analytic approach under the assumption that the non-radial component of the velocity is negligible. For our A-series runs, this assumption was not valid. In that series, we set the lateral velocities of the fluid to zero above the shock during a short time after bounce for numerical reasons, which led to a coherent deflection of collapsing matter when passing through shock, with a sudden and commensurate change in the -velocities of the fluid elements. One can see in Figure 2 the effect is more pronounced for a lesser progenitor mass. This happens because the relative contribution of the lateral velocity to the total velocity of the fluid is higher for less-massive progenitors (and, therefore, with lower radial velocities). In the B-series models, asymmetries in the angular velocities above the shock are obtained given commensurate asymmetries in the gravitational potential. This, in turn, reduces the jump in the angular velocities across the shock and excludes the presence of the coherent deflections seen in the A-series models and described above, as illustrated in Figure 2.
As was correctly pointed out in Müller et al. (2013), prompt convection cannot be the only source of the quasi-periodic signal in this emission phase, due to the difference in time scales of prompt convection (30 ms) and the prompt signal (80 ms). After prompt convection has ceased, we do observe a diminishing but nonzero signal amplitude. The reason is that the shock expands quickly during the first 80 ms after bounce. Therefore, the perturbed matter is accumulated in the fast-growing volume behind the shock. Although convection has become less pronounced after 20 ms, integration over an increasing volume in part compensates for this.
Further clarification of the contributions to the prompt GW signal would require simulations with a finer grid resolution that would be capable of capturing all hydrodynamic instabilities (i.e. prompt convection, turbulent cascades, acoustic and vorticity waves, etc.) that are presented in this phase.
The stalling of the shock manifests itself in a relatively short quiescent phase, which lasts about 20–30 ms and which is followed by a strong signal produced by the development of neutrino-driven convection and the SASI.
iv.3 Strong Signal Phase
The beginning of the strong signal phase coincides with the onset of SASI activity. It has been shown in previous studies Murphy et al. (2009); Marek et al. (2009); Yakunin et al. (2010) that the strong signal is actually produced by the combined effect of SASI-induced downflows impinging on the PNS surface and the subsequent deceleration of the matter at the PNS surface and the convection inside the PNS. The low-frequency component arises from the modulations in the shock radius as the SASI develops and evolves. The high-frequency component is generated when the SASI-induced accretion flows strike the PNS surface (Figure 3). It is clear from the analysis of the contributions to the strain from km and km that the PNS convection, deceleration of the accreting matter at the PNS surface, and neutrino-driven convection in the gain region contribute significantly.
The shock modulations affect the kinetic energy of the accretion flows and, consequently, the amplitude of the GWs generated when these flows hit the PNS surface. The signal structure during the strong signal phase in both B12-WH07 and B15-WH07 is similar to that in the corresponding A-series models. However, this is not the case for B25-WH07 and A25-WH07. The beginning of the strong signal phase in A25-WH07 is 50 ms behind that in B25-WH07, which indicates an earlier development of neutrino-driven convection and SASI activity in the latter model. The peak amplitude in B25-WH07 is twice as large as it is in A25-WH07.
iv.4 Explosion Phase
All of our GW signals end with a slowly increasing tail, which reflects the (linear) gravitational memory associated with accelerations at the prolate outgoing shock. The noticeable decrease of the high-frequency component of the amplitude during the explosion phase (most pronounced for model B12-WH07 at 520 ms) is due to the cessation of active accretion onto the PNS surface (Figure 4). The time of the cessation coincides, within a width of the STFT window, with the time when the frequency reaches its maximum value, for all of our models except B20-WH07 (Figure 1). B20-WH07 has a different explosion morphology. A single downstream is formed in all of our models except B20-WH07 in the early SASI phase. This downstream produces the local large amplitude spikes in the GW strain by its deceleration at the PNS surface. The downflow also induces the l=2 mode of the mass distribution deep in the PNS, which enables high-frequency PNS convection to contribute to the GW signal. Thus, PNS convection is responsible for the high-frequency component of the GW waveform. Termination of the single accretion stream leads to a significant decrease in both the frequency and the amplitude of the GW signal. In B20-WH07, multiple downstreams are formed during the SASI phase. This prevents the establishment of a more precise correlation between the changes of the accretion flow and the associated changes of the waveform amplitude and peak frequency. The typical frequency in B20-WH07 starts to decrease when the first accretion downflow detaches from the surface of the PNS (500 ms) while other downstreams continue to perturb the PNS and thus support the high-frequency and the amplitude of the B20-WH07 signal (Figure 5), until the moment when the last accretion down flow becomes detached from the PNS surface (630 ms).
After the cessation of accretion, the GW signal in all of our models is essentially generated by the shock only. The tails continue to rise until they reach their saturation values at 700–1000 ms, depending on the model and its prolateness.
The total emitted GW energy is shown in Figure 6. The values of the GW energy emitted in the B-series models presented here are very close to what we predicted in the A-series models presented in Yakunin et al. (2010). Due to the “anomalous”evolution of model B20-WH07, we do not observe a simple correlation between the progenitor mass and the total energy emitted in gravitational waves. That is, the GW energy emitted is not solely dependent on the progenitor mass. It is also a function of the explosion dynamics – in particular, the number and characteristics of the accretion streams that form during the pre-explosion and explosion phases. The GW energy emitted does increase monotonically with progenitor mass for models B12-WH07, B15-WH07, and B25-WH07, which share the same explosion morphology, but the results are very different for B20-WH07 given the difference in its explosion morphology and the resultant difference in the evolution of its accretion streams.
As shown in Figure 6, almost all of the GW energy is emitted between 200 ms and 700 ms after bounce for all of our models, and we do not observe significant contributions to in any model after 700 ms, when the low-frequency component of the GW signal becomes dominant. The jumps in the emitted gravitational wave energy correspond to abrupt increases in the accretion rate onto the PNS surface. This is easily seen by correlating these jumps with the counterpart spikes in the gravitational waveforms in Figure 6 that are the direct result of such accretion. Our predictions for the gravitational wave energy emitted are 2–3 times higher than those based on the general relativistic models G11.2 and G15 of Müller et al. (2013). This is largely due to the fact that the high-amplitude, GW tail contributes significantly to the GW energy emitted. In turn, such large-amplitude tails are not produced in models that do not explode robustly.
iv.5 Signals Produced by Neutrino Emission
The GW signals from neutrino emission in the B-series models are similar to the signals in their A-series counterparts, with some variation associated with the nonlinear stochastic nature of multidimensional supernova models. The amplitudes of all of the GW signals from neutrino emission are slightly negative just after bounce, until 180–220 ms, depending on the model, and then increase dramatically, becoming positive throughout the rest of the simulation. This is the result of the formation of a stable accretion down flow in the central region of the grid () due to an active interplay between neutrino-driven convection and the SASI at this time. The cold dense matter in the formed down flow absorbs neutrinos more efficiently than the matter in the polar regions. As a consequence, the neutrino luminosity is more intense in the polar regions, which makes the amplitude of the GW signal positive (Eq. 13). The situation is more intricate in B20-WH07, due to the presence of multiple down streams, but the general trend is similar to the other models. Note that the amplitude of the neutrino-generated GW signal is much larger than the amplitude of the matter-generated GW signal; however, neutrino-induced GW signals have relatively low frequencies ( Hz) for the canonical setup of current gravitational wave detectors. Nevertheless these signals may be detectable using the “non-traditional” approach presented in Christodoulou (1991); Bieri and Garfinkle (2013): three-mass experiments may allow one to measure a permanent displacement of the test masses due to the (linear) memory effect of gravitational waves.
iv.6 Detectability of the Signals
Figure 7 compares the GW strain spectra of our models with the broadband design noise levels of advanced-generation GW interferometers, assuming a source distance of 10 kpc. Most of the detectable emission is within 100–800 Hz, with the level increasing from (2 to 10) Hz. A Galactic event (at 10 kpc) appears to be well detectable by the upcoming generation of detectors. The peaks at 550–750 Hz are due to a cumulative effect of high-frequency convection inside the PNS and the deceleration of downflows at the PNS surface. In general, the peak frequencies of all of our models presented here are lower than those seen in the A-series models because of the low-frequency contribution of the late signal ( 600 ms). Though all of the peaks lie in a relatively narrow frequency interval, one can see that the peak frequency tends to decrease with increasing progenitor mass.
Our GW predictions for the B15-WH07 model can be compared to the M15 model of Müller et al. (2013) given that both groups implement similar treatments of the neutrino transport and GR corrections to the gravitational field, and include essentially the same physics in their models. The two groups are in agreement with regard to the time scales of the different (pre-explosion) GW phases, and the amplitude of the prompt and strong GW signals. They differ, however, in their predictions for the peak in the GW spectrum, which is at 1000 Hz in the M15 model versus 650 Hz in model B15-WH07. This difference likely arises due to the presence of a strong explosion in our simulation that considerably decreases active accretion onto the PNS after 400 ms post bounce and, consequently, the peak frequency of the GW signal (Figure 7).
V Summary and Conclusions
Based on four ab initio axisymmetric explosion models Bruenn et al. (2014) for non-rotating progenitors with masses 12, 15, 20, and 25 M, we studied the GW signals of core collapse supernovae from the early post-bounce phase through the fully-developed explosion phase. Unlike in our earlier studies Yakunin et al. (2010), which were truncated at 500 ms after bounce, here we provide the complete (up to 1 s) gravitational waveforms for all four models. This is the first time complete signals have been computed in the context of ab initio explosion models. This is particularly important for the signatures in frequency space, whose accurate determination requires a full temporal evolution.
Our models qualitatively confirm the four-phase picture of GW emission seen in our previous studies, and by others using parameterized models, with an early quasi-periodic signal, a quiescent phase of several tens of milliseconds, a strong stochastic GW signal lasting until some fraction of a second after the onset of explosion, and a low-frequency tail.
Given that we tracked the full dynamical and GW evolution beyond 1 s after bounce, we were able to follow the transitions between the four stages of the GW signal and, in particular, between the last two stages, at the moment of cessation of active accretion onto the PNS surface. This is clearly seen in the gravitational waveforms, both in the behavior of the strain as a function of time and in the evolution of the peak frequency of the GW signal, and is especially manifest in the B12-WH07 model. The evolution of the peak frequency of the signal, which declines monotonically after accretion has stopped, is clearly evident in all four cases. Moreover, the peak frequency in the GW energy spectrum and the characteristic strain is inversely related to progenitor mass. On the other hand, the total GW energy emitted does not exhibit a simple correlation with progenitor mass. For models B12-WH07, B15-WH07, and B25-WH07, which all exhibit the same prolate explosion morphology, the GW energy emitted increases monotonically with progenitor mass. However, model B20-WH07, with its more spherical explosion, emits significantly less energy in GWs than models B25-WH07 and B15-WH07, which indicates that the energy emitted in GWs is a gross function of two parameters: progenitor mass and explosion morphology.
Our findings clearly demonstrate that a complete prediction of gravitational waveforms and spectra is possible only for a ab initio simulation with a fully developed explosion. Both the peak frequency of the GW signal and the GW energy emitted depend on the duration of the GW signal. In the latter case, the GW energy emitted does not saturate until 400–700 ms after bounce, depending on the progenitor.
In addition to carrying out our simulations past 1 s after bounce, differences between the signals provided here and those published in our earlier work Yakunin et al. (2010) were obtained for the early, first-phase signal and, as discussed here, were the result of different model specifications – in particular, constraining the pre-shock flow to be spherically symmetric or not. The results described here were obtained in models that do not impose such a constraint, which is artificial.
A major shortcoming of the work presented here is our imposition of axisymmetry. Complete GW waveform predictions, including both the and polarizations, in the context of state-of-the-art three-dimensional supernova simulations are required. The expected differences in the stellar core hydrodynamics in three dimensions case Nordhaus et al. (2010); Burrows et al. (2012); Janka et al. (2012); Hanke et al. (2013); Murphy et al. (2013); Dolence et al. (2013); Couch (2013); Ott et al. (2013); Takiwaki et al. (2014); Fuller et al. (2015); Radice et al. (2015); Couch and Ott (2015) will have an impact on the predicted waveforms. In particular, changes in the geometry of the accretion down flows and the behavior of turbulence may influence the amplitude and energy of the GW emission. We have already reported a successful development of supernova explosion in the 3D Chimera simulation Mezzacappa et al. (2015). Within a month, we will present an overview of the simulation Lentz (2015) followed by the paper presented the 3D gravitational waveforms.
In addition to the leap to three dimensions, other “dimensions” of the problem – e.g., the use of different nuclear equations of state, progenitors (especially non-spherical progenitors (see Arnett and Meakin (2011)), etc. – need to be considered, as well, in the context of late-time three-dimensional models.
This research was supported by the U.S. Department of Energy Offices of Nuclear Physics and Advanced Scientific Computing Research; the NASA Astrophysics Theory and Fundamental Physics Program (grants NNH08AH71I and NNH11AQ72I); and the National Science Foundation PetaApps Program (grants OCI-0749242, OCI-0749204, and OCI-0749248). P. M. is supported by the National Science Foundation through its employee IR/D program. The opinions and conclusions expressed herein are those of the authors and do not represent the National Science Foundation. The authors would like to acknowledge fruitful discussions with Nelson Christensen.
Appendix A Tensor Spherical Harmonics
In this appendix, we write explicitly the tensor spherical harmonics. We follow the notation of Kotake et al. (2007).
a.1 Explicit Form of and
In general, the and functions are defined by
where is the usual scalar spherical harmonics of order and degree .
For (quadrupole approximation), we have the following explicit expressions:
a.2 Tensor Spherical Harmonics
Let us define the tensor spherical harmonics (in the -frame) using the and functions
Here the first row (column) corresponds to (), and is a normalization factor. Notice, this tensor is trace-free, and the diagonal components correspond to the mode, while the off-diagonal components correspond to the mode.
The normalization is fixed by the following relation:
where , and the metric on the 2-sphere, , is
The normalization factor for is .
- Originally, the stress-energy tensor contains not only the matter contribution but also the gravitational pseudo-tensor, which can be omitted in the linearized theory.
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